
Citation 
 Permanent Link:
 http://ufdc.ufl.edu/UFE0041972/00001
Material Information
 Title:
 Magnetism in nanoscale materials, effect of finite size and dipolar interactions
 Creator:
 Das, Ritesh
 Place of Publication:
 [Gainesville, Fla.]
 Publisher:
 University of Florida
 Publication Date:
 2010
 Language:
 english
 Physical Description:
 1 online resource (96 p.)
Thesis/Dissertation Information
 Degree:
 Doctorate ( Ph.D.)
 Degree Grantor:
 University of Florida
 Degree Disciplines:
 Physics
 Committee Chair:
 Hebard, Arthur F.
 Committee Members:
 Takano, Yasumasa
Biswas, Amlan Kumar, Pradeep P. Norton, David P.
 Graduation Date:
 8/7/2010
Subjects
 Subjects / Keywords:
 Anisotropy ( jstor )
Coercivity ( jstor ) Domain walls ( jstor ) Magnetic fields ( jstor ) Magnetism ( jstor ) Magnetization ( jstor ) Magnets ( jstor ) Nanoparticles ( jstor ) Particle interactions ( jstor ) Temperature dependence ( jstor ) Physics  Dissertations, Academic  UF dipolar, magnetism, nanomagnetics, nanomagnetism
 Genre:
 Electronic Thesis or Dissertation
bibliography ( marcgt ) theses ( marcgt ) government publication (state, provincial, terriorial, dependent) ( marcgt ) Physics thesis, Ph.D.
Notes
 Abstract:
 Material physics is always motivated by the materials with exotic properties. It was a common belief that exotic properties are only associated with exotic materials. Now it is clear that geometrical confinement at nanoscale dimensions can give rise to exotic properties even in simple materials. Ferromagnetic materials in restricted dimensions are extremely interesting because of their potential applications as well as the rich fundamental science involved. Magnetic nanoparticles are useful in high density magnetic data storage devices, sensors, contrast agents in MRI, drug delivery, treating hyperthemia and many more. All the applications of nanomagnets are very crucial in modern day life. But most of the applications are restricted due to the limitations in the fundamental properties arises in nanoscale and also due to the technical limitations of controlling things at nanoscale. For example particles become superparamagnetic as the size is reduced below a certain value and the magnetization direction fluctuates randomly due to the thermal energy which limits the density of data storage. The promises of nanomagnets are huge and to really achieve the grand challenges in nanomagnetism, it is necessary to understand the basic sciences involve at small scales. In this present work, the magnetic properties of systems in nanoscale (nanoparticles and thin films) have been investigated. The effect of dipolar interactions, particle size, particle size distribution, temperature, magnetic field etc. on the magnetic properties have been studied. ( en )
 General Note:
 In the series University of Florida Digital Collections.
 General Note:
 Includes vita.
 Bibliography:
 Includes bibliographical references.
 Source of Description:
 Description based on online resource; title from PDF title page.
 Source of Description:
 This bibliographic record is available under the Creative Commons CC0 public domain dedication. The University of Florida Libraries, as creator of this bibliographic record, has waived all rights to it worldwide under copyright law, including all related and neighboring rights, to the extent allowed by law.
 Thesis:
 Thesis (Ph.D.)University of Florida, 2010.
 Local:
 Adviser: Hebard, Arthur F.
 Electronic Access:
 RESTRICTED TO UF STUDENTS, STAFF, FACULTY, AND ONCAMPUS USE UNTIL 20110831
 Statement of Responsibility:
 by Ritesh Das.
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 Embargo Date:
 8/31/2011
 Resource Identifier:
 004979732 ( ALEPH )
705931020 ( OCLC )
 Classification:
 LD1780 2010 ( lcc )

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600 \ H
S Linear Fit of Data7_B
500 
0) 400
0
300 
200 U
5 10 15 20 25 30
d(nm)
Figure 65. He vs. d of Fe films at 10 K. Coercive field increases with decreasing d. This
behavior is due to fact that K increases with decreasing d which is very
common in multidomain thin films when the domain wall thickness is
comparable or larger than the film thickness. The domain wall thickness of
iron is about 60 nm,3 which is larger than the thickness of the films studied
here.
magnetic thin films when the domain wall thickness is comparable to or higher than the
film thickness.7 The domain wall thickness of iron is about 60 nm,3 which is larger than
the thickness of the film studied here. Note that we have used the value of K in Eq. 63,
which is larger than the bulk value. From Eq. 64, we find that v2 ~ 0.12.
6.5 Conclusion
The coercive field of multidomain Fe thin films has been investigated. The temperature
and thickness dependence of the coercive field agrees well with the prediction made by
Neel, which takes in to account the effect of free poles on the coercive field that occurs
at the small inclusions. The contribution of strain to the coercivity is very small for the
case of Fe and the dominant contribution comes from the free poles at the inclusions. The
volume fraction of inclusions has been estimated from the coercive field data to be around
0.12.
6
Step 1, 2, 3, 4 and 5 should be repeated for different particle size to determine the
MH loop for a given value of T for a sample consisting of nonuniform particle size
and random orientation of the easy axis of magnetization. In real samples the particle
distribution function is usually lognormal or gaussian.9'10
7
Step 1, 2, 3, 4, 5 and 6 should be repeated for different T to determine the
temperature dependence of the MH loop.7
8
Completion of step 7 will provide an opportunity to determine the temperature
dependence of the coercive field, remanent magnetization etc. Some of the temperature
dependent of coercive fields are listed in Tablel1.
Figure 18. continued
Magnetization loops at different temperatures for a single l .r sample of Ni nanoparticles
of average diameter around 18 nm are shown in Fig. 19. The coercive field is determined
by the magnetic field where magnetization changes sign and passes through zero. It is
clear from the Fig. 19 that coercive fields decreases with increasing temperature as
discussed above. At temperatures high compared to the anisotropy energy KV, the
magnetization directions can rotate freely over the barrier and the particles become
superparamagnetic with H=0. In this case the system can be treated similar to the case
of paramagnetism with each particle as a giant or super spin of value M1. V (thus called
CHAPTER 6
COERCIVE FIELD OF FE THIN FILMS AS THE FUNCTION OF TEMPERATURE
AND FILM THICKNESS: EVIDENCE OF NEEL DISPERSE FIELD THEORY OF
MAGNETIC DOMAINS
6.1 Abstract
The temperature dependence of the coercive field of Fe thin films has been investigated.
Three different samples of different thickness are studied. The coercive field decreases with
temperature and follows the same temperature dependence as the first order anisotropy
constant. This behavior is consistent with the theoretical prediction made by Neel15
based on the disperse field theory of magnetic domain which takes in to account the effect
of free poles on the coercive field that occurs at small inclusions. The value of coercive
field increases with decreasing film thickness. This behavior is expected for multi domain
ferromagnetic systems at nanoscale where the domain wall thickness is comparable to or
larger than the film thickness.
6.2 Introduction
The most interesting aspect of ferromagnetism is the hysteresis loop,90 which refers
to the history dependent behavior of magnetization with applied magnetic field (Fig. 62).
Hysteresis is a complex nonlinear, nonequilibrium and nonlocal phenomenon, reflecting
the existence of anisotropyrelated metastable energy minima separated by fielddependent
energy barriers.3 An extrinsic property of crucial importance in permanent magnetism is
the coercive field, the magnetic field where magnetization changes sign as it passes through
zero. The coercive field basically describes the stability of the remnant state and is a
very important concept for most practical applications.9199 Coercivity in ferromagnets
is known from very long time. 90 But, due to the complex nature, the origin of coercive
field is still a subject of study. In this present work the behavior of coercive field of three
different iron thin films with different thicknesses has been investigated. The temperature
dependence of the coercive field agrees well with the theory of domain wall pinning arising
OT OT
Omin
Figure 17.
At finite temperature other 0 values around min, will be occupied with a finite
probability according to the Boltzmann factor and shown by the shaded
region. The thermal average of the magnetization will be the average of the all
magnetization directions over this shaded region.7 The probability of having
some magnetization direction will be determined by the Boltzmann factor.
1
Start with the energy of the single particle.
E(H) =2KV l(si 2 0) cose
2
Find the minima of E(H)
S..VCosOi, will be the magnetization at T=0 for the given value of H, and V
Figure 18. Flow diagram to show the process of calculating coercive field for real
nanoparticle samples with particle size distribution and random orientation of
the easy axis of magnetizations at finite temperature.
kBT
43. Rojas, D. P., Barquin, L. F., Fernandez, J. R., Espeso, J. I., and Sal, J. C. G. Size
effects in the magnetic behaviour of TbAl_2 milled alloys. Journal of Ph,; 
Condensed Matter 19(18) (2007).
44. Tenzer, R. K. Influence of particle size on coercive force of barium ferrite powders.
Journal of Applied Ph;,. 34(4), 1267 (1963).
45. Zhang, T., Li, G., Qian, T., Qu, J. F., Xiang, X. Q., and Li, X. G. Effect of particle
size on the structure and magnetic properties of La_0.6Pb_0. \!iO_3 nanoparticles.
Journal of Applied Ph;. 100(9), (1,' :24 (2006).
46. Kittel, C. Physical theory of ferromagnetic domains. Reviews of Modern Ph;,i
21(4), 541583 (1949).
47. Stoner, E. C. and Wohlfarth, E. P. A mechanism of magnetic hysteresis in
heterogeneous alloys. Philosophical Transactions of The Royal S .:. /;/ of London
Series AMathematical and PI,;'..al Sciences 240(826), 599642 (1948).
48. Das, R., Gupta, A., Kumar, D., Hoh, S., Pennycook, S. J., and Hebard, A. F.
Dipolar interactions and their influence on the critical single domain grain size of
Ni in 1li, ,1 Ni/Al_20_3 composites. Journal of Ph ;,. .Condensed Matter 20(38)
(2008).
49. Neel, L. Ann. G(e 1~,;I 5, 99 (1949).
50. Neel, L. Proprietes magnetiques des ferrites ferrimagnetisme et
antiferromagnetisme. Annales De P,;;',.;,': 3(2), 137198 (1948).
51. Wohlfarth, E. P. The effect of particle interaction on the coercive force of
ferromagnetic micropowders. Proceedings of the Ph,; .. l '.'. .'. I of London
232(1189), 208227 (1955).
52. ElHilo, M. Effects of array arrangements in nanopatterned thin film media. Journal
of Magnetism and Magnetic Materials 322(912), 12791282 (2010).
53. Sharif, R., Z!i Ii X. Q., Shamaila, S., Riaz, S., Jiang, L. X., and Han, X. F.
Magnetic and magnetization properties of CoFeB nanowires. Journal of Magnetism
and Magnetic Materials 310(2, Part 3), E830E832 (2007).
54. Holmes, B. M., N. i.111 1i1 D. M., and Wears, M. L. Determination of effective
anisotropy in a modern particulate magnetic recording media. Journal of Magnetism
and Magnetic Materials 315(1), 3945 (2007).
55. ElHilo, M. and Bsoul, I. Interaction effects on the coercivity and fluctuation field in
granular powder magnetic systems. Pt,;,'..:. BCondensed Matter 389(2), 311316
(2007).
LIST OF FIGURES
Figure page
11 SD and MD particle ............... ............. 13
12 Coherent and incoherent rotation ... ............ ..... .. 14
13 Single particle in magnetic field ............... ........ ..15
14 Two state energy ............... ............ .. .. 16
15 Hysteresis of SD particle ............... ........... ..18
16 Diagram of a particle .................... 20
17 Thermal average of magnetization .......... .. 21
18 Flow diagram .................. .................. .. 21
19 MH below TB .. ..................... .. ..24
110 M H below TB ....... ....... .... ..... .. 25
111 SD to MD transition and He .................. .......... .. 26
112 Magnetization loop for MD particle .................. ..... .. 27
113 Domain wall and He .................. .............. .. 28
114 M vs. T for 3 nm Ni nanoparticles .................. ..... .. 30
21 STEM image of Ni particle .................. ........... .. 34
22 H, vs. d, different T .................. ............ .. .. 35
23 d, vs. T ................................ .. .... 37
24 Hd and domain ............... ............... .. 41
31 Sample ..... ........... ... .............. 45
32 MH loop. .................... ....... ...... .. ... 46
33 He vs. d: dipolar interaction .................. .......... .. 47
34 Dipolar interaction .................. .. 49
41 Physical and magnetic view of sample .................. ...... 53
42 Saturation magnetization vs. x .................. ........ .. 54
43 Coercive field vs. x .................. ............... .. 55
Figure 16. Single particle in an applied magnetic field (H). k is the direction of the easy
axis of magnetization. M and H are the magnetization and magnetic field
vectors respectively. Without loosing any generality M and H can be
considered in the same plane. The angle between M and H is 0. The angle
between H and k is Q. The energy barrier for this general configuration is
given by Eq. 116.7
MH loops for all possible i should be calculated. Averaging over all these MH loops will
give a magnetization loop at temperature T for a sample of uniform particle size and a
randomlyoriented easy axis of magnetization. All the above procedures should be done for
all possible particle sizes as the real samples usually have some particle size distribution.
The probability of a particular particle size can be modeled either as a lognormal or
gaussian distribution function. In this way the magnetization loop of a real sample with
nonuniform particle size and random orientation of the easy axis of magnetization can be
determined. If the all the above procedures are repeated for different temperatures then
the magnetization loop at different temperatures can be determined. Below we show a flow
diagram for the above process.79
Taking the second order derivative of Eq. 15, it can be shown that the Eq. 19 (Eq.
110) refers to minima (maximum) of the energy. Thus the energy minima are at 0 = 0
and 0 = 7 and maximum at when cosO=. [. 1/2K (see Fig. 14). Energies correspond to
these extrema are
Emi, = i [..VH (111)
Emin, = .VH (112)
Ema, = KV 1 + (f4[)] (113)
2K
where Emin, and Emin, corresponds to 0 = 0 (spin up) and 0 = 7 (spin down) respectively.
It is now easy to show that E+(H)= Emax Emin, and E_(H)= Emax Emin are given by
Eq. 16.
The energy barrier has to be overcome to reverse the magnetization direction from up
to down or vice versa. Brown proposed that this process requires a finite time5
r oexp E ( ) (114)
( kBT )
where T is the temperature, 71 is the inverse attempt frequency of overcoming the energy
barrier and kB is the Boltzmann constant.
Figurel5 shows the magnetization process when the magnetic field is swept from a
large positive value to a large negative value and again from a negative to positive value
to complete the magnetization loop. When magnetic field is large (scenario 1) all particles
will be magnetized along the magnetic field and a positive saturation magnetization is
achieved. As magnetic field is reduced to zero (scenario 2) the magnetization direction will
be trapped in the up direction as the temperature is not enough to overcome the energy
barrier. Now as the magnetic field is reversed the energy barrier, E_(H) will be reduced
according to Eq. 16 (scenario 3). But still the temperature is not enough to overcome
the energy barrier and the magnetization will still be trapped with a positive value. A
further increase in magnetic field in the opposite direction will keep lowering the energy
2 1. 
Different theoretical approaches concentrate on the derivation of (dW/dx)max.
Substantial wall motion may require fields of tens or hundreds of Oersted. Evidently
real materials contain crystal imperfections of one sort or another which hinder the easy
motion of domain walls. These hindrances are generally of two kinds: inclusions and
residual microstress.2
From a magnetic point of view, an "inclusion" in a domain is a region which has a
different spontaneous magnetization from the surrounding material, or no magnetization
at all. According to the result obtain by Neel in his disperse field theory (which basically
calculates the term (dW/dx)max), coercivity is given by Eq. 63 below.15
1 A2a2 Kv2
H, = v + (63)
4 K, 1. 11.
The first term is due to the residual microstress and vl is the volume fraction of the free
pole at the residual microstress and A, a, K and i.., are the saturation magnetostriction,
internal stress, magnet' il ii.1_,i. anisotropy constant and saturation magnetization
respectively. The second term in Eq. 64 originates due to the poles at the inclusions of
volume fraction v2. For iron, i1., = 1743 emu/cm3,2 K=8x106 ergs/cm3,101 A 10xt06102
and a=1010 dynes/cm2.103 Putting these values in the Eq. 63 we obtain,
H, 0.18vl + 46002 Oe (64)
Thus in our case the coercive field will be dominated by the 2nd term in Eq. 63,
which is proportional to K and agrees well with the experimental results as shown in Fig.
63 and Fig. 64. Remember that i.., is constant.
In Fig. 65 the variation of H,(d) is shown. The increase in H, with decreasing film
thickness, d, could be due to the enhancement of K with decreasing d.101,104,105 The
increase in coercive field with decreasing thickness is well known for the multidomain
14  Hc
4
Set 2
12 0
E *
2
o 10 t
10 Set 2
Set 1
8
Set 3 0
Dipolar interaction strength
Figure 34. Coercive field (He) and critical diameter (de) as the function of the increasing
dipolar interaction. H, (de) increases (decreases) with increasing dipolar
interaction. The opposite behavior of He and d, , r. I that the collective
dynamics and the critical slowdown is responsible for the increase in H, due to
the dipolar interactions. The decrease in d, is discussed elsewhere.48
observations (Fig. 34). Note that in this case the anisotropy energy is unaffected by
dipolar interactions and the increase in relaxation time is due to the fact that the reversal
of magnetization is collective in nature.64,65
3.4 Conclusions
A study of dipolar interactions is presented for the single and muiiltil i structure of
Ni nanoparticles. The coercive field has been found to increase with increasing dipolar
interactions and can be understood qualitatively in terms of collective dynamics.
Three sets of samples are investigated. Each set consists of samples having particle
size varying from 3 nm to 60 nm in diameter. Dipolar interactions are stronger in set 1
and decreases for set 2 and set 3. Behavior of coercive field and critical single domain
radius are observed. Coercive field increases and critical single domain radius decreases
Set 1
Set 3
*dc
o 40 2
400 200 0 200 400
20 H(Oe)
10 20 30 40 50 60
x(A)
Figure 43. The coercive field He shows a strong increase as the thickness x of the top
V, r of the Pd decreases. The data are shown as solid black circles and the
black solid line is a power law fit with exponent Tl 2.3(0.1). The inset
shows magnetization loops at T 10 K for x 8A (solid black squares) and
x 56A (solid red circles).
the number of Fe atoms present, the saturated magnetization i = 1.1 x 104emu/cm2
corresponds to 9.2 fi per Fe atom, in close agreement with previous observations
of the giant moment of Fe in Pd to be near 10 PB72. Modeling the x dependence of
i (x) shown in Fig. 42 for our Pd/Fe/Pd trilhv'ir is not straightforward. For regular
ferromagnets with if., uniform throughout the thickness, we would expect if. ,(x) to be
linear in x; clearly it is not. A reasonable model will incorporate an exchange interaction
J that decays radially with the distance from the point ferromagnetic impurity84. This
complication requires modeling J as a function of distance x from the plane of impurity. A
starting point would be to write the magnetization M is a function of J4,
M(H, T, x) i= 1. 8, PBH + 2pMJ(x) (41)
\kBT
where 'erfi' is the imaginary error function, i. ., is the saturation magnetization, /
KV/kBT and a = V(3cos2 l)/s3 is a dimensionless parameter with and s
corresponding respectively to an angle parameter and the separation between two .idi i:ent
particles each with volume V The parameter Q is alv,v greater than one for T < TB
where there is still coercivity; i.e., the magnetization is fluctuating but not going over
barriers. Then Eq. 21 has the limiting value at T > 0 as given below.
Hd T T 0 (22)
47
The derivation of Eq. 21 includes averaging over the accessible directions of
magnetization weighted by a Boltzmann factor. Higher temperatures give smaller
magnetizations since the particles fluctuate over larger angles. Specifically, spin up
and down particles will be in energy minima separated by an anisotropy energy barrier.
At absolute zero temperature only the direction corresponding to the minima of the
energy will be occupied. At finite temperatures, according to the Boltzmann law, other
energy states will be occupied around this minimum and will have different directions
of magnetizations. Thus to obtain the actual magnetization, an average over all these
accessible directions is calculated, constrained by the fact that the probability of those
states to be occupied is given by the Boltzmann factor
OT exp E(0)
OTep[ ( ]'( '
fK exp[ f]dO
where at zero magnetic field E(O) =KVsin20 Thus Omin = 0 and OT is temperature
dependent, obeying the relation, sin20T = kBT/KV The parameter OT (see Fig. 17 on
page 21 of chapter) will be higher at higher temperatures and thus the thermal average of
the magnetization will diminish at higher temperatures. Using Eq. 23 one can determine
the temperature dependence of the dipolar magnetic field Hd as shown in Eq. 21 for
particles treated as simple dipoles.
minima. As the temperature is increased the spins can hop over the energy barrier to
reach the global minima. Due to this trapping of spins in local minima, magnetization
values depends strongly on the cooling protocol. There are mainly two different cooling
protocols, field cooled (FC) and zero field cooled (ZFC). The behavior of magnetization
as a function of temperature for the two protocols is shown in Fig. 114 below for the
sample of Ni nanoparticles of 3 nm diameter at an applied field of 20 Oe. The temperature
where the difference between FC and ZFC disappears is generally called the irreversible
temperature (Ti,). For nanoparticles Ti, is same as the blocking temperature (TB).2
1.5x10 0 Im
FC H = 20 Oe
1.0x10 
i/4
5.0x10^ 
ZFC
0.0
0 50 100 150 200 250 300
T(K)
Figure 114. Magnetization vs. temperature at an applied magnetic field of 20 Oe for the 3
nm diameter Ni nanoparticles. The red color is the field cooled (FC)
magnetization and the black one is the zero field cooled (ZFC) magnetization.
1.4.1 Zero Field Cooled (ZFC) Magnetization
Zero field cooled magnetization is measured by cooling the sample from high
temperature (temperature above the irreversible temperature (Tir)) without any applied
magnetic field. At low temperature a small magnetic field is applied and magnetization
is measured as a function of temperature during the warm up while keeping the magnetic
field on. Here we will discuss the shape of the ZFC magnetization in a qualitative manner.
In general the magnetic system can be treated as a twostate problem as shown previously
that with increasing temperature this upper bound to particle size increases and then
saturates due to attenuated dipolar interactions from thermally induced coherent motions
of the magnetization of the neighboring randomly oriented particles.
2.3 Experimental Details
The composite system studied in this paper comprises elongated and pi li, iv H11i.'
Ni particles with diameters in the range of 360 nm embedded as lvir in an insulating
A1203 host. The muiltiliv r samples were fabricated on Si(100) or sapphire (caxis)
substrates using pulsed laser deposition from alumina and nickel targets. High purity
targets of Ni (99.9' '. ) and A12O3 (99.9'" .) were alternately ablated for deposition. Before
deposition, the substrates were ultrasonically degreased and cleaned in acetone and
methanol each for 10 min and then etched in a I!' I'_ hydrofluoric acid (HF) solution to
remove the surface silicon dioxide lv,_, thus forming hydrogen terminated surfaces.35
The base pressure for all the depositions was of the order of 10' Torr. After substrate
l., lii. the pressure increased to the 10Torr range. The substrate temperature was kept
at about 550" C during growth of the A1203 and Ni 1 .ir. The repetition rate of the laser
beam was 10 Hz and energy density used was ~ 2 Jcm2 over a spot size 4 mm x 1.5 mm.
A 40 nmthick buffer li;vr of A12O3 was deposited initially on the Si or sapphire substrate
before the sequential growth of Ni and A1203. This procedure results in a very smooth
starting surface for growth of Ni as verified by high resolution scanning transmission
electron microscopy studies (Fig. 21). Multill , samples were prepared having 5 1 ,ris
of Ni nanoparticles spaced from each other by 3 nmthick Al20s3 1I ,r. A 3 nmthick cap
l ,r of A1203 was deposited to protect the topmost l1*ir of Ni nanoparticles.
Shown in Fig. 21 is a crosssectional TEM image from a multi1 i,, 1 (5 l.. rs)
NiA1203 sample grown on cplane sapphire. The Ni particles have a size of 23 5
nm in width and 9 nm in height. The separation between neighboring particles is on
the order of 3 nm (measured as a projected distance in crosssectional view), which
is comparable to the thickness of the A1203 spacer l iVt. For the purposes of this
Alumina
Ni particles
Substrate
Set 1 Set 2 Set 3
Figure 51. Schematic of three sets of samples. Set 1 comprises a single lIr of Ni
particles embedded in an A1203 matrix. Set 2 and Set 3 comprises of 5 1l.ri
of Ni particles separated by different distances in an A1203 matrix. The
interlayer distances in Set 2 and Set 3 are 3 nm and 40 nm respectively.
with a general magnetic energy landscape of the system written as a polynomial expansion
of the domain wall position (x) around a strong pinning center.24,6
E(x) = ao + aix + a2x2 + :3 boHx (52)
2 3
where ao, al, a2, a3 and bo are micromagnetic parameters that depend on the magnetic
parameters K, ., and A. For the strong pinning center the x3 term is included as the
effect of the pinning center is long distance compared to the weak pinning center where
the x3 term is neglected.3 The relation between micromagnetic and magnetic parameter
can be determined from the particular model used. Note that the micromagnetic
parameters are temperature independent in our case as they only depend on the
temperature independent magnetic parameters. First, we will derive the energy barrier
separating the metastable minima from the global minima. The maxima or minima of
E(x) are determined by setting the first order derivative to zero.
E
= at + a2x + a3X 2 boH = 0 (53)
6x
4w4w4w
IM IMIM
40 4040
56000 K
Linear Fit of Data4 C
54000
52000
50000
48000
380 400 420 440
H (Oe)
Figure 64. H, vs. K of Fe film of thickness 9 nm. The linear behavior ii I the
validation of Neel's disperse field theory of magnetic domains which takes in to
account the effect of free poles on the coercive field that occurs at small
inclusions (Eq. 63). The similar behavior is observed for other two samples
which is expected as they have similar temperature dependence.
Theories concerned with the coercivity of the multi domain ferromagnetic materials
begin with the consideration of the change in magnetic energy across a domain wall.2
Since the magnetization changes from [ ., to I .. across a 180 domain wall, the effective
pressure on the wall will be the difference in the energy across the wall per unit volume.
At an applied magnetic field H, the pressure will be 2H.1 .. Thus the work done to move
a domain wall of area s to a distance dx will be2
dW 2H.1[.sdx (61)
The above equation can be generalized for any angle (not only 180") domain wall.2
The term dW/dx, which is basically the energy required to move a domain wall to unit
distance, is the measure of the resistance of domain wall motion.2 In real samples due to
impurities, imperfections or irregularities in crystal, dW/dx passes through maximum and
minimum. The origin of reversibility in the magnetization loop is the irreversible motion of
domains through these maximum and minimum. 2 The coercive field is usually calculated
using the equation below.2
TABLE OF CONTENTS
page
ACKNOW LEDGMENTS ................................. 4
LIST OF TABLES ....................... ............. 8
LIST OF FIGURES .................................... 9
A BSTRA CT . . 11
CHAPTER
1 THEORY AND BACKGROUND ................... ..... 12
1.1 Single Domain and Multi Domain Particles ....... .......... 12
1.2 Hysteresis Loop of Single Domain Coherently Rotating Particles ...... 14
1.3 Hysteresis Loop of Multi Domain Particles ................. .. 24
1.4 Magnetization vs. Temperature .......... .. .. .. 29
1.4.1 Zero Field Cooled (ZFC) Magnetization 30
1.4.2 Field Cooled (FC) Magnetization ..... 31
2 DIPOLAR INTERACTIONS AND THEIR INFLUENCE ON THE CRITICAL
SINGLE DOMAIN GRAIN SIZE OF NI IN LAYERED Ni/A120O COMPOSITES 32
2.1 Abstract .. .. .. .. ... .. .. .. ... .. .. .. .. ...... .. 32
2.2 Introduction .................. ................ .. 32
2.3 Experimental Details .................. ........... 33
2.4 Data and Discussion .................. ........... .. 36
2.5 Conclusion .. ..... .. 40
2.6 M ethods .................. .................. .. 41
2.6.1 Mathematical Analysis .............. .. 41
2.6.2 Basic Physical Understanding ............... .. .41
3 EFFECT OF DIPOLAR INTERACTION ON THE COERCIVE FIELD OF
MAGNETIC NANOPARTICLES: EVIDENCE FOR COLLECTIVE DYNAMICS 42
3.1 Abstract .................. .................. .. 42
3.2 Introduction .................. ................ .. 42
3.3 Results and Discussions .................. ......... .. 44
3.4 Conclusions .................. ................ .. 49
4 FINITE SIZE EFFECTS WITH VARIABLE RANGE EXCHANGE COUPLING
IN THINFILM Pd/Fe/Pd TRILAYERS .................. ..... 51
4.1 Abstract .................. .................. .. 51
4.2 Introduction .................. ................ .. 51
4.3 Experimental Details .................. ........... .. 52
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on magnetic properties of ultrafine ferromagnetic particles. P;,';.. ,'l Review Letters
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30. Hansen, M. and Morup, S. Models for the dynamics of interacting magnetic
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31. Jonsson, P. and GarciaPalacios, J. Relaxation time of weakly interacting
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34. Morup, S. and Tronc, E. Superparamagnetic relaxation of weakly interacting
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Synthesis and atomiclevel characterization of Ni nanoparticles in Al_20_3 matrix.
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Ph;,. 9(8), 12671269 (1976).
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and electrical properties of the solgel prepared Li_0.5Fe_2.50_4 fine particles. Journal
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40. Jiang, J. and Yang, Y.M. Facile synthesis of nanocrystalline spinel NiFe_20_4 via a
novel soft chemistry route. Materials Letters 61(21), 42764279 (2007).
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singledomain particles. Journal of Applied Ph;,.. 34(3), 656& (1963).
42. Luna, C., Morales, M., Serna, C., and Vazquez, M. Multidomain to singledomain
transition for uniform Co_80Ni_20 nanoparticles. Nano'.. 1,,,,1. ,.i; 14(2), 268272
(2003).
*4
o10 
E
5)
< 8 MsA (Fe)= 2.63x105 emu/cm
I
6 I
0 10 20 30 40 50 60
x(A)
Figure 42. The saturation magnetization normalized to the area of the sample if i shows
a smooth increase with increasing thickness x. The experimental data are
shown as solid black circles and the dashed black line is a guide to the e,
Saturation to a constant value occurs near 30A (vertical arrow).
4.4 Results and Discussion
For large values of x, the thickness y of the combined polarized ferromagnetic Pd
1~..i~ and the associated saturated magnetization M = I ., will reach a constant value.
This expectation is borne out in Fig. 42 which shows the xdependence of saturated
magnetization i. i normalized to sample area. We note that this normalized saturated
magnetization i [. (x) increases with increasing x as the total amount of polarized Pd
increases. The onset of saturation, near x = 30 A indicates that the polarization cloud
including the embedded Fe lir is ~ 60 A thick. This value is consistent with previous
observation73. The increase of if.. with x shown in Fig. 42 is thus straightforward to
understand. As x increases the thickness of the top polarized ferromagnetic Pd lv1r
increases with a concomitant increase of magnetic material in the system. Variation of x
clearly controls the thickness of the polarized ferromagnetic Pd l1~Vr. When normalized to
16. Bates, L. F. and Martin, D. H. Domains of reverse magnetization. Proceedings of the
Pi,;,.. ,' S I,; Section A 66(2), 162 (1953).
17. Babonneau, D., Petroff, F., Maurice, J., Fettar, F., Vaures, A., and Naudon, A.
Evidence for a selforganized growth in granular Co/Al_20_3 miiltilhi ris. Applied
Ph;,i. Letters 76(20), 28922894 (2000).
18. Jamet, M., Wernsdorfer, W., Thirion, C., Mailly, D., Dupuis, V., Melinon, P., and
Perez, A. Magnetic anisotropy of a single cobalt nanocluster. P,;;.,. al Review Letters
86(20), 46764679 (2001).
19. M.inii., H., Nakatani, I., and Furniib z,hi T. Phase transitions of ironnitride
magnetic fluids. P,;,.:. ,,l Review Letters 84(26), 61066109 (2000).
20. Puntes, V., Krishnan, K., and Alivisatos, A. Colloidal nano. ivi iI shape and size
control: The case of cobalt. Science 291(5511), 21152117 (2001).
21. Stamm, C., Marty, F., Vaterlaus, A., Welch, V., Egger, S., Maier, U., Ramsperger,
U., Fuhrmann, H., and Pescia, D. Twodimensional magnetic particles. Science
282(5388), 449451 (1998).
22. Sun, S., Murray, C., Weller, D., Folks, L., and Moser, A. Monodisperse FePt
nanoparticles and ferromagnetic FePt nano. ivi 1I superlattices. Science 287(5460),
19891992 (2000).
23. Skumryev, V., Stov iii., S., Z! iir. Y., TH ilij.ianayis, G., Givord, D., and Nogues, J.
Beating the superparamagnetic limit with exchange bias. Nature 423(6942), 850853
(2003).
24. Selrinv.r, D., Yu, M., and Kirby, R. N i ructured magnetic films for extremely
high density recording. Nanostrctured Materials 12(58, Part B Sp. Iss. SI),
10211026 (1999).
25. Andersson, J., Djurberg, C., Jonsson, T., Svedlindh, P., and Nordblad, P. Monte
Carlo studies of the dynamics of an interacting monodispersive magneticparticle
system. PI,;,.:. a Review B 56(21), 1398313988 (1997).
26. Dormann, J., Bessais, L., and Fiorani, D. A dynamic study of small interacting
particles superparamagnetic model and spinglass laws. Journal of Ph;,.. CSolid
State Ph ;. 21(10), 20152034 (1988).
27. Dormann, J., DOrazio, F., Lucari, F., Tronc, E., Prene, P., Jolivet, J., Fiorani, D.,
C('! : I ii R., and Nogues, M. Thermal variation of the relaxation time of the
magnetic moment of gammaFe_20_3 nanoparticles with interparticle interactions of
various strengths. P/,;. ,,al Review B 53(21), 1429114297 (1996).
28. Elhilo, M., Ogrady, K., and C'!i i1l ell, R. Susceptibility phenomena in a fine
particle system .1. concentrationdependence of the peak. Journal of Magnetism and
Magnetic Materials 114(3), 295306 (1992).
O
0 0.5
0.4
0.3
0.2
0.1
0.0
0 10 20 30 40 50
T2/3 (K2/3)
Figure 55. Coercive field (He) vs. T2/3 for five different samples of set 3. The linear
behavior is observed for samples with particle size from 16 nm to 44 nm in
diameter.
5.4 Relation Between Micromagnetic Parameter and Magnetic Parameters
Here we will outline a roadmap to relate the micromagnetic parameters ao, al, a2,
a3 and bo to the magnetic parameters K, ., and A. To do that we will start with the
magnetic energy expression,3
E(x) = A (v ( ))2 K(x)(k.M())2 oM(x).H M(x).Hd(M) dV
(512)
where the first term corresponds to the exchange energy cost due to the spin misalignment,
the second term is the anisotropy energy, the third term is the Zeeman energy and the
fourth term is the magnetostatic self energy. The position of the domain wall is given by x
and k is the unit vector along the easy axis. The above equation should be solved for real
H
Figure 13. A SD particle in an applied magnetic (H) field along the easy axis of
magnetization (k). 0 is the angle between the magnetization M and the easy
axis k.
of the energy occurs at 0 = 7/2 separating the two energy minima. Figurel4 a) shows
the energy diagram at zero magnetic field as a function of 0. In this case the particle will
have magnetization parallel to the easy axis of magnetization since these correspond to
minimum energy states (up or down). Any other directions will cost some anisotropy
energy. The two states with minimum energy are separated by the anisotropy energy
barrier equal to KV. In an applied magnetic field along the easy axis the two energy
minima will be shifted due to the Zeeman energy (Fig. 14 b) ). Now the state along the
magnetic field will be most stable as the energy is lowered due to the Zeeman term. The
state with opposite direction of magnetization will be metastable. The magnetic field
dependent energy barrier for the spin up (E+(H)) and down (E_(H)) state is calculated
by Stoner and Wohlfarth to be,6
E(H)= KV 1 (16)
where E+(H) is the energy barrier seen by the up magnetized particles and E_(H) is the
energy barrier seen by the down magnetized particles and Ho = 2K/M, .. Derivation of the
Eq. 16 is given below.
0 50 100 150 200 250 300
T(K)
b)
300
S200
U
100
0
4 5 6 7
T'2K)
Figure 71.
Irreversible magnetization AM(H, T) defined as the difference of the FC and
ZFC magnetizations is a quantitative measure of hysteresis. a, Black squares
and red circles represent respectively the FC and ZFC temperaturedependent
magnetizations for sample A in a 20 Oe field applied parallel to the film
surface. The irreversible magnetization AM(H, T) is shown by the twoheaded
vertical dotted arrow. Inset: Large thermally blocked magnetic particles (1
and 3) with respective vertical and horizontal easy axes of magnetization
indicated by the arrows. Particle 2 is small enough to be superparamagnetic
(thermally unblocked). For magnetic fields applied along the vertical direction,
particles 2 and 3 do not contribute to AM(H, T). b, The coercive field (He)
for the same sample shown as a function of T1/2 (Blue stars) does not show
the linear behavior expected for ideal StonerWohlfarth particles6 where all the
particles are uniform size and aligned with the applied field (particle 1). The
solid blue line is a fit to the data using a lognormal distribution of particle size
together with a random orientation of the easy axis of the magnetizations.
Inset: Schematic magnetization curves for the cases where (bl) only particles
1 and 2 and (bl) only particles 1 and 3 are present. The resultant
magnetization loops (black curves) for the two cases show the pronounced
effects of particle size and easy axis orientation on the determination of H,.
are commonly accepted measures of hysteresis, the underlying phenomenology for each
is considerably different. For example in nanoparticle magnetic systems such as shown
in Fig. 71, AM(H, T) and Hc(T) are sensitive in different vo to both the presence of
superparamagnetic particles and the random orientation of the easy axis of magnetization
of each particle. The insets of Fig. 71 a) and b) schematically illustrate these differences
using three particles: particles 1 (red) and 3 (blue) with easy axes of magnetization
S5
0
 mFC
*ZFC
I I I
has been observed.3 P li. i lii, i11 1!: particles will therefore have crystalline grains
oriented in different directions, thus tending to average any net crystalline anisotropy
to zero. Accordingly, temperatureindependent shape anisotropy is dominant and
temperaturedependent (
important to note that the exchange length l,, = 14.6 nm for Ni,37 which is the length
scale below which atomic exchange interactions dominate over magnetostatic fields,
determines the critical radii (Rcoh) for coherent rotation: Rcoh ~ 51,, for spherical particles
and Rcoh ~ 3.51,, for nanowires.3 The particle sizes (1.530 nm in radius) that we have
investigated are thus smaller than the critical radius below which coherent rotation of Ni
prevails.
400
2001[
Figure 22.
0 20 40 60
Particle Size (nm)
Coercivity for 51,ir Ni/Al20 muiltil ,r samples (5 repeated units) plotted
as a function of particle size (diameter) at the temperatures indicated in the
legend. The peak positions at d = d, for each isotherm, indicated by vertical
arrows, delineate the crossover from single domain (SD) to multiple domain
(Ml1)) behavior (d > de). Inset shows the behavior of H, as a function of 1/d
for the particles with d > de at 10 K. The linear dependence up to 24 nm
diameter particles with saturation at a constant value for large par i !. is
consistent with the behavior expected for multidomain particles. Thus
particles on the righthand side of the peak are multidomain.
In Fig. 22 we show plots of H, as a function of particle size d at each of the
temperatures indicated in the legend. Coercive fields were extracted from magnetization
SD < > MD 45  H js. Id
10 K
24..r.
002 0.04 m0.6 0.00
lid(nm
l
S\100 K
Sr 1o K
'/ 4 15 K
2010 Ritesh Kumar Das
CHAPTER 1
THEORY AND BACKGROUND
Ferromagnetism is known for more than 2500 years to man. The first magnetic
material discovered was magnetite (Fe2O3). The practical applications of ferromagnets
was recognized from very ancient time. The first use of magnetic material was as a
compass. According to the magnetic properties, materials can be divided into diamagnetic,
paramagnetic, ferromagnetic, antiferromagnetic, ferrimagnetic, spinglass etc. In this
present work ferromagnetism will be the main topic. C'! lpters followed by this chapter
will discuss the effect of finite size and dipolar interactions on the magnetic properties of
some materials with nanoscale structures. In this chapter a general theoretical background
will be given.
1.1 Single Domain and Multi Domain Particles
When the size of the particle is very small, it will contain only one magnetic
domain. 13 This is because the energy required to form a domain is larger than the
magnetostatic self energy. The magnetostatic self energy for a spherical particle is given
by1
Ema, ,1 2V/12 (11)
where po is the free space permeability, i.. is the saturation magnetization and V is the
volume of the particle. The energy required to form a Bloch domain wall is13
Ed, 4= AKR2 (12)
where K is the anisotropy constant, A is the exchange stiffness and R is the radius of the
particle.
Note that Emag grows as R3 and Edw grows as R2. Domain formation is therefore
favorable for larger particles as the magnetostatic energy will be large compared to
the domain wall formation energy. The critical single domain radius (Rsd) where the
I dedicate this to my parents and family for their active support. Without them it would
have not been possible.
with increasing dipolar interactions. These two behaviors together si' I a collective
dynamics of the magnetization reversal process in the SD region in the presence of dipolar
interactions. To our knowledge, this is the first time that the effect of collective dynamics
on a coercive field of the nanoparticle system has been observed.
reverse the direction of the magnetization of a coherently rotating SD particle is given by
the relation2'5'49'50
T = Toexp (32)
kBT_
Here, To is the inverse of the attempt frequency to overcome the energy barrier, V is the
volume of the particle, kB is the Boltzmann constant and T is the temperature. Stoner
and Wohlfarth have calculated He for SD particles in the simple case when particles are
coherently rotating and the applied magnetic field is along the easy axis of magnetization
of the particles. The coercive field for a StonerWohlfarth particle is given by
2K I (ntr1n (2f
Hesw = 1 n ( (33)
where Tm is the time of measurement. From the simple StonerWohlfarth model it is clear
that He for the nanoparticle can depend on many different factors. He increases with
decreasing T,, increasing T and increasing K.
In the presence of dipolar interactions the above equation will be modified. The
widely accepted modification is achieved by treating the dipolar interactions to result in
an effective anisotropy energy.5161. Thus if due to the dipolar interactions K increases
(decreases) then ', according to Eq. 32, will also increase (decrease) and as a net result
He will increase (decrease). A more familiar famous form of Eq. 33 is Hsw(T) =
2K/M..(1 (T/TB)1/2), where TB = KV/25kB is the blocking temperature. The factor 25
comes from the fact that Tm, 100 s is a typical measurement time and rol ~ 109 sec1 is
a typical attempt rate.
The effect of dipolar interaction on the coercive field (He) has been investigated
extensively. The first theoretical treatment by Neel62 showed that He decreases with the
increase in the packing fraction (c) or the dipolar interaction as shown below in Eq. 34,
where the interaction effect has been introduced as an "Interaction Field" and shown to
barrier until, at the coercive field, the energy barrier can be overcome by the thermal
energy and magnetization reversal will occur (scenario 4). When H
4 3
Figure 15.
He the energy
2 1
Hysteresis of a coherently rotating SD particle. Scenario 1) High positive
magnetic field is applied and saturation magnetization is observed. Scenario 2)
Magnetic field is reduced from positive value to zero. Magnetization is trapped
in the positive direction as the thermal energy is not enough to overcome the
energy barrier. Scenario 3) Magnetic field direction is reversed. Still the energy
barrier is large compared to the thermal energy and magnetization is trapped
in the positive direction. Scenario 4) Magnetic field equals to the coercive
field. Now the energy barrier can be overcome by thermal energy and
magnetization reversal occurs.
barrier E_ (H) is such that the relaxation time 7
Tm at the temperature T. Where Tm
is the experimental measurement time (around 100 sec for SQUID measurement). Thus
when H= H, magnetization reversal occurs. Combining Eq. 16 and 114, the coercivity
(He(T)) of the SD particle can be calculated as shown below.
7 = Tm= oexp E_(H)BT
\kBT
= E (H,)
kBTln T
To
V VMT Sr .y FePt nanoparticles (6 nm)
0 2 4 6
H/Hm
Figure 74. Scaling collapse describes irreversible magnetization (hysteresis) in a wide
variety of ferromagnetic materials. a, Plots of the reduced irreversible
magnetization AM(H, T)/AMlma(T) as a function of reduced magnetic field
H/H,(T) for the six different magnetic materials labeling each curve. The
implicit temperature variable increases from left to right and each color on a
given curve represents a different AM(H, T) isotherm. For clarity, the ordinate
values have been shifted and the solid lines have been added as guides to the
eye. The bottommost curve for single crystal spinglass Cu:Mn (at. 1.5 .)
material is taken from the literature6
for magnetic ordering together with a wide range of materials properties. The scaling
collapse applies equally well: to single domain (SD) coherently rotating Ni nanoparticles
with average particle diameter of 3nm embedded in an insulating matrix; to multidomain
(l 1)) incoherently rotating Ni nanoparticles with average particle diameter of 12 nm also
embedded in an insulating matrix; to coherently rotating uniform size FePt nanoparticles
(6 nm diameter); to continuous metallic Gd thin films with magnetization derived from
local moments supplemented by band structure exhibiting some itinerant character; and
to mixedphase manganite (LPC'\ 10) where the Mn spins order by a double exchange
mechanism in an environment where chargeordered and paramagnetic insulating phases
compete with a ferromagnetic metallic phase. We have also included a spin glass material,
single crystal Cu:Mn (1.5 at ), described in the literature1l6. The collapse occurs for
nanoparticle systems which include SD, MD and superparamagnetic particles with both
I am indebted to my parents for their support, encouragement and for alvi
believing in me. I appreciate the warmth and affection of my sister Mridula. I could not
have come this far without their blessings.
in Fig. 14 where spin up and down correspond to the energy minima separated by some
energy barrier. The origin of the energy barrier in the SD case is the anisotropy whereas
for the case of MD the origin is domain wall pinning at defects. At high temperature the
energy barrier is easily overcome due to the thermal energy and the spin up and down
states will be equally populated. Thus at high temperature above Ti,,, magnetization will
be zero. Now if the sample is cooled to a low temperature without any applied magnetic
field, then zero magnetization state will be blocked as the energy barrier is now large
compared to the thermal energy.2,3,6 If a small magnetic field is applied the change in
magnetization will occur only for the small energy barriers that can be overcome at that
temperature and a small magnetization will be achieved. As temperature is increased, the
probability of overcoming the larger barriers increases and magnetization increases. At
temperature Tir the probabilities to overcome the barrier for spin up and down become
nearly equal and the spin up and down mixing starts to happen and thus magnetization
decreases with further increase in temperature.
1.4.2 Field Cooled (FC) Magnetization
Field cooled magnetization is measured by cooling the sample from high temperature
to the low temperature in an applied magnetic field and magnetization is measured during
the warm up process.2 In this case at high temperature due to the applied magnetic field,
the spin up states are more populated than the spin down states. Cooling the sample at a
low temperature while keeping the field on will thus lock the system in magnetized state.
An increase in temperature will increase the probability of spin up and down mixing and
thus magnetization will gradually decrease.
K is anisotropy constant).3 Values of A (oc ,,,, 1' ) and B (oc A,,K ) have been found
to be 1.44 x 104Jm3 and 1.21 x 10lJm2 respectively. This value of A is very close to
the theoretical predicted value3 and the value of B is again consistent with the value
of the shape anisotropy. The value of the shape anisotropy can also be predicted from
the zero temperature extrapolation H,, ~ K/M1. for randomly oriented particles.3 For
Shape = 3.1 x 104Jm3, H,, ~ 620 Oe. This is in good agreement with the 500 Oe coercive
field observed at 10 K for the 6 nm sample.
For a separate series of single livr samples the coercivities at 10 K peak at de
S14 nm as shown in Fig. 23 by the blue star. In the single lvr samples the peak
position occurs at higher particle size (14 nm) than muiltiliv r samples (8 nm). This
difference reinforces our interpretation and can be understood by realizing that the
dipolar interactions of the single 1 ir samples are significantly reduced compared to the
rniitil i.r samples because of the smaller number of nearest neighbors.
2.5 Conclusion
In summary, we have fabricated magnetic nanoparticles in an insulating thin film
matrix with tunable properties achieved by varying particle size and temperature.
The peaks in the coercivity isotherms delineate a critical grain size de which identifies
the crossover from SD to MD behavior. The presence of dipolar interactions and
their diminishing influence with increasing temperature is responsible for the observed
dependence of de on temperature and is in good qualitative agreement with our modification
of present theory26 of interacting particles. The wellestablished influence of dipolar
interactions on superparamagnetic relaxation time2534 together with the connection
between relaxation time r and coercivity H, sil. 1 that there is a concomitant influence
of dipolar interactions on the coercivity observed near the superparamagnetic limit where
He = 0. The work reported here extends this connection to the upper limits on the size
of SD particles by showing that dipolar interactions can facilitate the formation of multi
domain particles especially at low temperatures.
with fixed thickness y/2 would have a Tc equal to the highest T, of the top livr. In this
case the overall measurement would not show a strong change in T, as a function of x,
since the T, of the bottom l?vr would dominate for all x.
We note that for our planar geometry, Tc decreases with decreasing thickness as has
also been shown for thinfilm Nisl and epitaxial thinfilm structures based on Ni, Co
and Fe82. On the other hand T, increases with decreasing size of ferrimagnetic MnFe204
nanoscale particles with diameters in the range 526 nm83. This increase of T, with
decreasing size is attributed to finite size scaling in three dimensions where all three
dimensions simultaneously collapse83. In our twodimensional planar thin films only one of
the dimensions, the thickness, collapses and T, decreases rather than increases in accord
with the observations of previous studies81'82
4.5 Conclusions
In conclusion, we have characterized the magnetic properties of thinfilm Pd/Fe/Pd
tril1vis and determined that critical size effects apply to I! iiii ;iwtic" Pd where the
ferromagnetism is induced by proximity to an underlying ultra thin Fe film. The critical
size, or equivalently the critical thickness, is controlled by varying the thickness x of
the top Pd l~.vr. The dependence on film thickness of the coercive field He and the
Curie temperature T, are in qualitative agreement with finite size effects seen in regular
ferromagnetic films where the exchange coupling J is constant throughout the film. The
results presented here increase our understanding of nanomagnetism in ultra thin systems
by showing that the spatial variations of J in the proximity coupled Pd have a pronounced
influence on the form of thicknessinduced variations, namely: a nonlinear dependence
of I.[. (x), an unusually strong powerlaw dependence of H (x) and a dependence of
T,(x) which indicates that the trilayer acts as a single l1v.r that necessarily includes the
constant thickness Pd l?vr serving as a substrate for the Fe 1l.r.
magnetization (Mr) will be seen at zero magnetic field. Reversing the magnetic field will
IH
II
Figure 112.
I I
Hysteresis loop of a MD system and possible domain wall configuration. At
very large positive magnetic field all the spins are aligned along the magnetic
field and saturation magnetization is achieved. When magnetic field is
reduced to zero, a domain wall forms. Due to the imperfections in the
sample, the domain wall will be stuck in a position such that the up domain
is larger than the down domain and remanent magnetization is measured. If
the direction of the magnetic field is reversed the domain wall will start to
move to the right and the down domain will grow. At a magnetic field equal
to the coercive field, the down and up domain will be equal in size and
magnetization will be zero. For a large negative magnetic field the domain
wall be moved to the right and all the spins will be in the direction of the
magnetic field and negative saturation will be reached.
move the domain wall to the right side and thus the down domain will start to grow and
magnetization will be reduced. When the negative magnetic field is equals to the coercive
field the up and down domain will have same size and magnetization will be zero. Further
increase in magnetic field in the negative direction will force the domain wall to move all
the way to right making all spins aligned along the magnetic field and negative saturation
will be reached.
* M
M S/
LIST OF TABLES
Table page
11 H, vs. T ...... ........... ............... .. .. 29
MAGNETISM IN NANOSCALE MATERIALS, EFFECT OF FINITE SIZE AND
DIPOLAR INTERACTIONS
By
RITESH KUMAR DAS
A DISSERTATION PRESENTED TO THE GRADUATE SCHOOL
OF THE UNIVERSITY OF FLORIDA IN PARTIAL FULFILLMENT
OF THE REQUIREMENTS FOR THE DEGREE OF
DOCTOR OF PHILOSOPHY
UNIVERSITY OF FLORIDA
2010
from small inclusions (for example
free pole is not negligible. 15
impurity or vacancy defects) where the energy of the
6.3 Experimental Details
Figure 61. TEM image of Fe thin film of thickness 9 nm.
Thin films of Fe were fabricated on Si(100) and sapphire (caxis) substrates using
pulsed laser deposition from alumina and iron targets. High purity targets of Fe (99.9' .)
and A1203 (99.9'.) were alternately ablated for deposition. Before deposition, the
substrates were ultrasonically degreased and cleaned in acetone and methanol each for 10
min and then etched in a 49'. hydrofluoric acid (HF) solution to remove the surface silicon
dioxide l ir (for the Si substrates only), thus forming hydrogen terminated surfaces.35
The base pressure for all the depositions was of the order of 107 Torr. After substrate
1i. lii. the pressure increased to the 10Torr range. The substrate temperature was
kept at about 550" C during growth of the A1203 and Fe lv ir. The repetition rate of the
laser beam was 10 Hz and energy density used was ~ 2 Jcm2 over a spot size 4 mm x
1.5 mm. A 40 nmthick buffer livr of A12O3 was deposited initially on the Si or sapphire
substrate before the sequential growth of Fe and A1203. This procedure results in a very
E
Figure 14.
At t
Solu
0 7 0 7
Two state energy of a SD particle. Two energy minima correspond to the
direction of the easy axis of magnetization. a) At zero magnetic field the
particle will have magnetization along the easy axis of magnetization as those
correspond to minimum energy states (up and down). Up and down states are
separated by the energy barrier equal to KV. To reverse the magnetization
direction from up to down or vice versa the system has to overcome the energy
barrier.5 Brown proposed that this process requires a finite time given by Eq.
114.5 b) In an applied magnetic field along the easy axis, the two energy
minima will be shifted due to the Zeeman energy. Now the up state which is
along the applied magnetic field will be most stable and have the lowest
energy. The state with opposite direction (down state) of magnetization will
be metastable. The magnetic field dependent energy barrier for the spin down
state is calculated by StonerWohlfarth (Eq. 16) 6
First order derivative of Eq. 15 with respect to 0 is
JE(H) 2KVsin0cos0 + i1 ..VHsinO
60
he maxima and minima
2KVsin0cos0 + i1 ..VHsinO 0
tions of the above equation are
sin0 0
cosO
(17)
(18)
(19)
(110)
i 2K
2K
CHAPTER 3
EFFECT OF DIPOLAR INTERACTION ON THE COERCIVE FIELD OF MAGNETIC
NANOPARTICLES: EVIDENCE FOR COLLECTIVE DYNAMICS
3.1 Abstract
The effect of dipolar interaction on the coercive field is discussed for the single
domain and coherently rotating Ni nanoparticles embedded in A1203 matrix. Results
for two sets of 5 livr samples with different interlayer spacing and a set of single l1ir
samples of Ni nanoparticles are compared. The dipolar interactions are strongest in the
samples with shorter interlayer distances and weakest for the single 1ivr samples. In
this present study, the dipolar interaction is found to increase the coercive field. On the
other hand the critical single domain radius decreases due to the dipolar interactions.
These two behaviors together indicate that collective dynamics pl i', an important role in
understanding the origin of the coercive field.
3.2 Introduction
The origin of coercive field (H,) for coherently rotating ferromagnetic nanoparticles is
remarkably different than that of the bulk,47 where irreversible domain wall motion is the
dominant mechanism.4 In the case of nanoparticles, when the size of the particle is smaller
than a critical size (dc), the most favorable energy state is to have single magnetic domain
and particles are called single domain (SD) particles. When H, is plotted as a function of
particle diameter (d), there is a well defined peak at de. Particles with d < d, (d > d,) are
SD (multidomain (I\l))). 2,8,41,42,44,48 Kittel3,46 has shown that for a spherical particle, d, is
given by the relation (see Eq. 13 on page 13 of chapter)
dc 72 (31)
S' ,, /.'
where A is the exchange stiffness, K is the anisotropy constant, /o is the free space
permeability and [.. is the saturation magnetization. In SD particles there is no domain
wall. The origin of H, in this case is the finite time required to reverse the magnetization
direction over the magnetic field dependent anisotropy energy.47 The time required to
barrier that arises due to strong domain wall pinning depends on the magnetic field with a
power of 3/2 and is responsible for the temperature dependence of the H,.
T to 5 T and again from 5 T to 5 T to complete the loop. At high magnetic fields the
magnetization from the Fe saturates and the magnetic field dependence arises due to the
diamagnetic contribution from the substrate. The diamagnetic contribution from the Fe
film is negligible as the thickness of the film is very small compared to the thickness of the
substrate. Thus the high magnetic field data is linear in magnetic field with a negative
slope. The slope of the line is determined from the linear fit of the high field data and
subtracted from the raw data to extract the ferromagnetic signal due to the Fe thin film.
The procedure is repeated for all samples and for all temperatures. The coercive field
is found to decrease with increasing temperatures. The results for all three samples are
presented in Fig. 63. Figure 64 shows the relation between K(T)s7 and H,(T) where
T is the implicit variable."7 The linear behavior of H, and K i r, I that the coercivity
mechanism is similar to the disperse field theory of magnetic domain which takes in to
account the effect of free poles on the coercive field that occurs at small inclusions. 15
600
S 99 nm
550 
500
450
8 400 
350 21 nm
300
250
25 30 nm
200  .
0 50 100 150 200 250 300
T (K)
Figure 63. H, vs. T of Fe films of thickness 9 nm, 21 nm and 30 nm. The temperature
dependence of all three samples is similar, which ir . i that the origin of the
coercive field depends on the intrinsic property of the iron, which in our case is
the magnetocrystalline anisotropy. This is true as for the case of extrinsic
origin the energy barrier depends on the size of the sample as discussed in
chapter 5
broad and uniform size distributions and magnetic moment reorientations arising from
complex superimpositions of domain wall motion and domain rotation which can be very
different in continuous films compared to nanoparticles where the extent of the domain
wall is comparable to the size of the particle. Thus the materials measured here are very
much different in terms of the origin of the irreversible magnetization.
In conclusion, we have presented a heretofore unreported phenomenological result
showing that the temperature and field dependent hysteresis of at least six distinctly
different magnetic systems can be collapsed onto single curves (Fig. 74) using the
particularly simple functional form expressed by Eq. 1. Our finding that such a scaling
collapse applies to magnetic systems totally different than the spin glass for which similar
scaling has been previously noted116'117 (the lowest curve in Fig. 74) t' I that
explanations116 relying on spin glass phenomenology are too narrow. Thus a more general
theory is needed to explain the scaling collapse. This collapse must imply an underlying
symmetry that is not captured by previous analytical and computational treatments and
may be a crucial clue to understand the complex history dependent magnetization process.
The similarity with the spin glass material is interesting and may be because of the fact
that all ZFC magnetization is a metastable state of the system and shows properties
varying with time. Thus the dynamics of the spins may pl. i a very important role for
the scaling collapse. The behavior of A/Mmax(T) is investigated for the 3 nm Ni particles.
We it'' 1 a new approach to investigate the magnetization reversal process from the
AAM,,x(T) measurement. We have successfully applied the method for the coherently
rotating SD particles.
7.4 Conclusions
In conclusion, we have presented a surprisingly general and unrecognized phenomenological
result showing that the temperature and field dependent hysteresis of at least six
distinctly different magnetic systems can be collapsed onto single curves (Fig. 74)
using the particularly simple functional form expressed by Eq. 1. We have not yet found
any exceptions. For the particularly simple case of coherently rotating single domain
particles (samples A and B), our analysis of scaling collapse bypasses the complications of
nonuniform size distributions and random easy axis orientation, unveiling an underlying
StonerWohlfarth behavior6. Our finding that the same scaling collapse more generally
applies to magnetic systems with a wide variety of mechanisms giving rise to hysteresis,
~i.' I that explanations116 relying on spin glass phenomenology are too narrow.
Thus a more general theory is needed to explain the scaling collapse. This collapse
must imply an underlying symmetry that is not captured by previous analytical and
computational treatments and may be a crucial clue to understand complex history
dependent magnetization processes. The similarity with the spin glass material116
is , ..,~ li' . and may be related to the fact that all ZFC magnetizations represent
metastable states of the system, which if given sufficient time would relax toward the
fieldcooled equilibrium state. Accordingly, the dynamics of the spins may pl iv a very
important role in understanding the scaling collapse.
7.5 Methods
7.5.1 Ni Nanoparticle.
Composite films comprising magnetic Ni nanoparticles embedded in an Al203 host
matrix were synthesized by pulsed laser deposition (PLD)36. High purity targets of Ni
(99.9' . ) and Al203 (99.99 .) were alternately ablated in the same deposition run. The
base pressure of the deposition was on the order of 10' Torr. The substrate temperature
was maintained near 550C during the growth. The repetition rate of the laser beam was
10 Hz and energy density used was 2 J cm2 over a spot size of 4 mm x 1.5 mm. A 40
nmthick buffer lvr of Al203 was deposited initially on the sapphire substrate before
the sequential growth of Ni and A1203. This procedure results in a very smooth starting
surface of growth of Ni as verified by the high resolution scanning transmission electron
microscopy (STEM) studies. Samples consists of 5 l' ,irs of Ni and Al203. A cap livCr
of A1203 was alvii used to protect the sample from oxidation. Zcontrast STEM image
0 100 200 300 400
H,(T) (From MH) (Oe)
Figure 73.
For single domain particles the ansatz AMmx(T) oc H,w is verified, a, The
linear dependence of AMmax(T) on T1/2 is in accordance with the
StonerWohlfarth theoretical prediction that Hc(T) oc T1/2 for the coherently
rotating single domain particles of sample A. The use of AMmax(T) rather
than H,(T) as a measure of hysteresis removes the effects of nonuniform
particle size and random orientation. b, The values of H,"I(T), computed for
uniform size FePt particles (sample B) from the ansatzderived Eq. 2 at the
indicated temperatures, scale linearly with HSW(T) which is determined from
the coercive fields of M H loops after correction for the random orientation
of the easy axis of magnetization (see Methods).
The scaling collapse behavior plotted for sample A in Fig. 72b si. , that AM has
the form,
AM(H, T) AM,,(T)F (H/H,(T)) ,
(71)
where F is an unknown function with the property F(1)
1. Taking the second partial
derivative of the both sides of this equation and solving for AMmax(T) gives the result:
(92F(h)F2 /h 2) 1 h 1H, T)a2 AM(H, T)/aH2 ,H(T) evaluated at the
hl 1mT
Slope 1.09(4)
10K
20 K
30 K
500 600
AMmC(T)
t tt t\ /
ttttt
Coherent rotation
/ttit 1t t
H H / t
Incoherent rotation
Figure 12. Coherent and incoherent rotation of the magnetization. In case of coherent
rotation all the spins rotate together and the whole particle can be considered
as a giant spin. Coherent rotation happens for SD particles with size smaller
than the exchange length lex
1.2 Hysteresis Loop of Single Domain Coherently Rotating Particles
The magnetization dynamics of the SD particles with R < lex will be coherent and the
particle can be treated as a giant single spin of value M MsV. When a magnetic field
(H) is applied along the easy axis of the magnetization (k) the energy of the particle is24
E(H) = KVsin20 i..VHcosO (15)
where 0 is the angle between the applied magnetic field and the direction of magnetization
as shown in the Fig. 13. The first term in Eq. 15 corresponds to the anisotropy energy
and the second term corresponds to the Zeeman energy. The energy, E(H), is shown
in Fig. 14 b) below as a function of 0 which shows two energy minima separated by
a barrier. The energy minima occur at 0 = 0 (corresponding to the magnetization
along the applied magnetic field or up direction) and 0 = 7 (corresponding to the
magnetization opposite to the applied magnetic field or down direction). The maximum
To derive the coercive field in MD domain case consider a simple case, as shown in
Fig. 113, where a single domain wall separates two domains. The right hand side is a spin
up domain and left hand side is a spin down domain. In an applied magnetic field, H,
Figure 113. Single domain wall separating two magnetic domains. Right hand side is a
spin up domain and left hand side is a spin down domain. In an applied
magnetic field due to the Zeeman energy the domain wall will experience a
pressure and some work need to be done to move the wall against this
pressure. The origin of hysteresis in MD sample is the irreversible motion of
the domain wall.
along the spin up domain, the Zeeman energy of the up (down) domain will be 1 I[
(+M I) per unit volume. Thus the energy difference across the domain wall will be
2HMs per unit volume. This energy difference can be considered as a pressure on the
wall and some work has to be done to move the domain wall against this pressure. The
work done to move the wall a distance dx is2,11
dW = 21. [Sdx (119)
where S the area of the domain wall. Thus the work done to move the wall by unit
distance is2,11
dW/dx = 21. IS (120)
CHAPTER 7
SCALING COLLAPSE OF THE IRREVERSIBLE MAGNETIZATION OF
FERROMAGNETIC THIN FILMS
7.1 Abstract
In ferromagnetic materials, hysteresis, or equivalently the history dependent behavior
of the magnetization, reflects complex nonlinear and non equilibrium phenomenology that
has been recognized for many years5'6'106108. Hysteresis depends strongly on materials
properties such as structural length scales spanning the nanometer to micrometer range3
and manifests complex behaviors including magnetic relaxation with aging dependence109
dimensionally dependent dipoledipole interactions48'110, spinglass like memory effects 1
and supermagnetism112. Here we show that the irreversible magnetization, defined as
the difference between fieldcooled and zerofield cooled magnetization, has a striking
similarity for a wide variety of ferromagnetic materials. This similarity becomes apparent
when the irreversible magnetization is normalized to its maximum value and plotted with
respect to a temperature dependent renormalized field. The collapse of the irreversible
magnetization onto a single curve for a given system implies an underlying symmetry to
hysteresis that is not captured by previous analytical3,'5'6'48,106,107'109112 and computational
treatments108s113 and thus provides a unifying theme that embraces a broad range of
complex hysteretic behavior.
7.2 Introduction
In general, hysteresis is a complex nonlinear non equilibrium phenomenon which
reflects the presence of fielddependent energy barriers between anisotropydependent
metastable minima. Accordingly, hysteresis is affected by a combination of intrin
sic properties such as magnetocrystalline anisotropy which depends on crystal field
energy and spinorbit coupling and extrinsic properties such as sample shape, grain
boundaries, disorder and imperfections. For example, in bulk ferromagnets hysteresis is
often described as a superimposition of domain wall motion and domain rotation with
energy barriers related to magneto' i i 1iiw., anisotropy together with imperfections
H(Oe)
0 2 4
H/Hm
Figure 72.
All of the data for AM(T, H) of sample A can, with proper normalization, be
made to collapse onto a single curve, a, Isotherms of AM plotted as a function
of H show selfsimilar behavior with maxima AMma,x(T) occurring at
characteristic fields Hm(T) marked by the vertical arrows. With decreasing
temperature AMmax(T) increases and H,(T) moves to higher fields. b, The
scaling collapse occurs when AM(H, T)/AMma,(T) is plotted against the
normalized field H/Hm(T). Inset: Plots of H, (squares) and H,(T) (stars) as
a function of T. The data and fit for H, are the same as shown in Fig. Ib, but
plotted with respect to T rather than T1/2. The solid line for Hm(T) is a guide
to the cv
SW behavior. The insensitivity of AM(H, T) measurements to superparamagnetic
particles and perpendicular orientations of blocked particles together with our ansatz
imply that more useful information about the magnetization reversal process is obtained
from AM(H, T) measurements than H,(T) measurements.
In
0
o
b) 1.0
0.9
0.8
56. Crew, D., Girt, E., Suess, D., Schrefl, T., Krishnan, K., Thomas, G., and Guilot, M.
Magnetic interactions and reversal behavior of Nd_2Fe_14B particles diluted in a Nd
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60. Kuo, P. C. and C('!, i C. Y. Effect of packing density on the coercivity of elongated
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68. Crangle, J. and Scott, W. Dilute ferromagnetic alloys. Journal of Applied Ph;;,., 36,
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69. Nieuwenh.GJ. Ferromggnetic transition temperature of dilute PdCo, PdFe and
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samples while taking into account real structure and imperfections. The real structure and
imperfections are responsible for the x dependence of the magnetic parameters (3 ..(x),
A(x), K(x)). After solving Eq. 512 and by comparing the coefficients of the different
power of x, it is possible to find out the micromagnetic parameters in terms of magnetic
parameters. The behaviors of H o and Eo/kB are shown in the figure below.
500
450
0
O 400
350
350
10 20 30 40 50 60
d (nm)
700
600
500 c
C)
LU
400
300
Figure 56. The behaviors of H o and Eo on particle diameter are shown for set 2 samples.
Ho decreases and Eo/kB increases with increasing particle size.
The increasing behavior of Eo and decreasing behavior of Hco are consistent with
the literature.3 The actual behavior can be very complicated as it depends on the real
structure factors and imperfections in the material.3
5.5 Conclusions
We have investigated the temperature dependence of the coercive field of MD Ni
nanoparticles in A1203 matrix. He decreases linearly with the T2/3. This behavior can be
understood according to the strong domain wall pinning. We show that the general energy
Set 2
 Hco
e EO/kB
2.6 Methods
2.6.1 Mathematical Analysis
The Eq. 25 is self consistent (as the term / contains dc) and can not be solved
analytically. The equation, d dco + dd w (ei(1 ), ))
w3ir(erfi~jQ I I 3P1)
0, is solved by numerical
approach and simultaneously the solution is fitted to the experimental data according
to a nonlinear list square method. Mathematica, a commercial software, is used for this
purpose.
2.6.2 Basic Physical Understanding
A simplified physical understanding of the problem is shown in Fig. 24.
1 1 Hd
\i\~s~ wy
Hd'
Figure 24.
The net effect of dipolar magnetic field (Hd) is shown on the particle 1. As
particles are randomly oriented, Hd from particle 3 will be in different
direction than that from particle 2. As dipolar interaction decreases rapidly
with distance, particle 1 will experience local dipolar magnetic fields in
different directions from different neighboring particles and thus making it
easy to form domains.
44 Curie temperature vs. x
51 Three sets of sample .
52 MH loops of set 2 .....
53 He vs. T2/3 set 1 samples
54 He vs. T2/3 set 2 samples
55 He vs. T2/3 set 3 samples
56 Hco and Eo of set 2 .
61 TEM image of Fe film .
62 MH loop of Fe film ..
63 He vs. T of Fe film .
64 He vs. K of Fe film ..
65 He vs. d of Fe film .
71 Irreversible Magnetization
72 Behavior of the AM(H, T)
73 The anstz .. .......
isotherms
as the function of
74 Scaling collapse of variety of ferromagnetic materials .. ............
and
scaling
collapse
Particle diameter
Figure 111. Coercive field plotted as a function of particle diameter. For very small
particles the coercive field is zero and the particles are known as
superparamagnetic particles (SP). As the particle size is increased the
coercive field increases due to the fact that the energy barrier increases.
Particles with size larger than the critical single domain radius are
multidomain and coercive field decreases with increasing particle size.
explains the behavior in Eq. 118. Thus the the peak in the coercive field when plotted
as the function of the particle size delineates the SD and MD behavior. In experiment we
have found the same behavior for both rmultil vr and single l r samples of Ni particles
in A1203 matrix as will be discussed in detail in chapter 2.
Figurel12 shows the possible domain wall configuration for different points in the
magnetization loop. Remember that compared to the SD case where the origin of the
hysteresis was the hopping over a energy barrier, in case of MD the origin of hysteresis is
irreversible domain wall motion. At very high magnetic field all the spins in the system
will be aligned along the magnetic field and positive saturation (. [.) will be achieved
(Fig. 112). As the magnetic field is reduced to zero a domain wall will be formed. Due
to the imperfections in the sample, the domain wall will be stuck in a position such
that the up domain is larger than the down domain and net magnetization or remanent
d
at \
10 K
3 nm separation (Set 1)
40 nm separation (Set 2)
Single layer (Set 3)

30 40
Figure 33.
Coercive field (He) as a function of particle diameter (d). The peak separates
the single domain (SD) and multidomain (\ l)) particles. Particles with
diameter higher (smaller) than the peak diameter (de) are MD (SD). Data for
the 3 different sample sets are shown and indicated in the legends. The critical
diameters d1,, dc2, d,3 are shown from the samples of set 1, set 2 and set 3
respectively. In the single domain region (below d,) the coercivity increases
with increasing dipolar interactions as shown by the vertical dotted arrow.
magnetization due to the dipolar interactions is found to be responsible for the increase in
He. These observations are shown in Fig. 33 and summarized in Fig. 34.
We first discuss the effect of dipolar interactions on He as presented in previous
investigations. 5161 The treatment begin by including the change in anisotropy energy Edrp,
due to dipolar interaction into the expression for r, as given by63
SKV + Ed ]
T7 Toexp L j
kL IT
(35)
600
400
0
o
200
0 10 20
d (nm)
d 0
ACKNOWLEDGMENTS
I am truly indebted to ri: irn: individuals who have contributed to the success of my
research work. Therefore, I express my sincerest regrets to any person not specifically
mentioned here.
First and foremost, I am thankful to my research advisor Prof. A. F. Hebard for
giving me the opportunity to work with him. It has been a great experience to work
under his supervision. His positive, openminded attitude toward research creates a unique
laboratory environment full of encouragement. I have learned a lot from his unadulterated
enthusiasm, willingness to learn and elegant but simple approach to understanding
fundamental physics.
I would like to thank all the present and former lab members for their helps and
pleasant ( ".'r. ir:. I am grateful to John J. Kelly for teaching me many experimental
techniques when I joined the group. Thanks to all the lab members Patrick, Rajiv, Sef,
Siddhartha, Sanal, Xiaochang for their helps. I really enjoi, d working with you guys.
I would also like to acknowledge the staffs of machine shop and electric shop.
Specially cryogenic staffs, Greg and John, for their constant supply of liquid He and
N2 all year around 24/7. Thanks to Jay (really a nice guy) for looking after all the pumps
and chillers.
I would like to thank all of my committee members. I will specially thanks Prof.
Amlan Biswas. Though I did not have chance to collaborate with him, but his guidance
and support towards my degree have been very helpful. I am also greatly thankful to Prof.
D. Norton for the wonderful collaboration and for letting me use his lab facilities.
I am thankful to my collaborators D. Kumar and A. Gupta from NCA&T. I am also
very thankful to Matt, Patrick, KyeongWon from Prof. Norton's lab for their helps and
being good friends.
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on critical phenomena in Ni films. Solid State Communications 14, 1075 (1974).
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structures. Reports on Progress in Ph;t,. 71, 056501 (2008).
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curietemperature in nanoscale MnFe_20_4 particles. P;;',..: Review Letters
67, 3602 (1991).
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We have investigated thinfilm Pd/Fe/Pd trial 'r;i in which the thickness dFe of the
Fe is held constant near 1.5A and the thickness of the polarized ferromagnetic Pd is
varied by changing the top Pd 1vr thickness x. The magnetic properties are studied as
a function of x. Our experiments are motivated by the recognition that ferromagnetism
in restricted dimensions has attracted significant research interest74 78. For example,
the coercive field He increases as the thickness of the ferromagnetic film is decreased
toward a thickness comparable to the width of a typical domain wall79'80. Moreover, the
Curie temperature T, decreases as the thickness of the ferromagnetic film is decreased
toward a thickness comparable to the spinspin correlation length8183. We will show
below that similar phenomenology applies to ferromagnetically polarized Pd films, albeit
with different functional dependence arising from the fact that exchange coupling, which
decays with distance from the ferromagnetic impurity84, is not uniform throughout the
film.
4.3 Experimental Details
The samples were grown on glass substrate by RF magnetron sputtering. The base
pressure of the growth chamber was of the order of 109 Torr. First a thick livr of Pd of
thickness 200 A is grown on top of the substrate. The root mean square surface roughness
of this Pd l1 r was measured by atomic force microscopy to be ~ 6 A. Then a very thin
(1.5 A as recorded by a quartz i I I1 monitor) lIvr of Fe is deposited on top of the
first Pd 1 i.r. Finally a top 1V.r of Pd with thickness x is grown to complete the trili vr
structure shown schematically in Fig. 4la. We discuss six different samples with the
top Pd 1~vr having a thickness x varying from 8 to 56 A. The total thickness y of the
polarized Pd (see Fig. 41b) can range from 20 to 100 A72,73. Thus for x < y/2, changes
in x will give rise to changes in y. Auger electron spectroscopy (AES) was used to verify
the presence of a well defined Fe l. r. The AES measurements were performed in a
1010 Torr vacuum at sequential intervals following removal of sub angstrom amounts
of Pd using an Argon etch. The depth profile of the high intensity Fe3 (703.0 eV) LMM
16 Simulation
Experiment
14 *
S12
S10 I I
8
6 I
0 50 100 150 200 250
T(K)
Figure 23. Peak position, d,, plotted as a function of temperature (red circles). The black
squares are the results derived from equation 25. The blue star represents the
observed value of dc for a series of single lwr samples at 10 K. The inset, a
schematic of three neighboring particles oriented in different directions,
illustrates how the dipolar fields from particle 2 and 3 facilitate the formation
of domains in particle 1, as the dipolar magnetic fields are in different
directions.
in the inset of Fig. 23. Particle 1 experiences dipolar fields from particles 2 and 3, which
are not collinear for most orientations of a randomly oriented particle system. Because
dipolar fields decrease rapidly with interparticle separation, the dipolar field due to
particle 3 (2) will be stronger than particle 2 (3) on the left (right) side of the particle 1.
The separate and unequal influence of the neighboring particles thus favors the formation
of domains in particle 1.
.To make these notions more quantitative, we modify the treatment of Dormann
et a126 for interacting paramagnets to include the temperature region below the blocking
temperature TB and find the temperaturedependent dipolar magnetic field Hd arising
from temperature induced fluctuations in the magnetization of nearest neighbor nanometer
size particles to be,
Hd .a eC(1 e) 1
47r v/j(erfi(3) erfi(v  T ))
Thermal average
(M(H, V))}T=
3
of the magnetization
SAE
f[2 Msvcosoexp 7BTde
AE
f02 exp ~WT d0
AE = Eo Eoin 01 and 02 are shown in Fig. 17
(M(H, p, V))T is the magnetization at temperature = T for the given value of H,
and V
Figure 18. continued
4
Step 1,2 and 3 should be repeated for different H. This will determine the MH loop
for a given value of T, b and V
5
Step 1, 2, 3 and 4 should be repeated for all possible b and average of all those loops
will determine the MH loop for a given value of T and V for an ensemble of particles
with random orientation of the easy axis of magnetization.
maximum where h(T) = H/Hm(T) = 1. The first term, (2F(h)/0h2) 1 h must be
a constant because of the scaling collapse. The remaining two terms have the same form
as the expected value of an effective anisotropy field114. Thus according to our ansatz,
AMmax(T) oc Hf we can write the relation
Hw(T) CH, (T)a2AM(H, T)/aH2 = CHf'(T), (72)
where C is a constant and Ha(T) = H2 (T)2 AM(H, T)/OH2 In (Tis computed from
experimental data.
To test the result expressed in Eq. 2, we use magnetization data on a system of
a;,,' .rm size (6 nm diameter) FePt nanoparticles (sample B, see Methods) synthesized
via thermal decomposition of Fe(CO)5 and reduction of Pt(acac)2115. The measured
coercive field HKH (T) is obtained from MH loops at different temperatures. Assuming
that the particles easy axes of magnetization are randomly oriented, a temperature
dependent correction to HfH(T) must be made so that HSW(T) can be inferred. This
correction is needed (see Methods) since the magnetization of randomly oriented uniform
size particles shows a T3/4 dependence7 compared to the T1/2 dependence expected for
an idealized sample in which all the particles are aligned along the applied magnetic
field. The plot of Fig. 73 includes this correction and shows a linear dependence of
Hcal( T) on HKH(T) as would be expected for a system of coherently rotating SD uniform
size FePt nanoparticles. The linear behavior with slope of 1.09(4) confirms the validity
of our model as expressed by Eq. 2 with C ~ 1. In Fig. 74 the reduced irreversible
magnetization, AM(H, T)/AMm,a(T), is plotted as a function of reduced magnetic
field, h(T) = H/Hm(T) for a wide variety of thinfilm magnetic materials labeled in
the inset and described in Methods. Unexpectedly, when plotted in this manner, the
magnetization data for each materials system collapse onto single curves which have
similar shapes described by a unique function F(H/Hm(T)) (see Eq. 1) for each system.
This data collapse is quite remarkable considering the variety of mechanisms responsible
is comparable to the domain wall thickness w79. For the case of Neel walls, He depends
only on the roughness of the film and does not depend on film thickness77. The variation
of Hc(x) becomes particularly pronounced when the film thickness becomes comparable to
w.
A qualitative understanding of the steeper H((x) dependence becomes evident by
recognizing that the formation of domain structure is driven by the reduction of long
range magnetostatic energy which at equilibrium is balanced by shorter range exchange
and anisotropy energy costs associated with the spin orientations within a Bloch or Neel
domain wall. Domain wall thickness is given by w = /A/K3'82 where K is the ii 1 H!iii
anisotropy constant and A is the exchange stiffness, proportional to the exchange energy,
Jss. The domain wall size w increases for decreasing K and increasing J. If K, which
depends on the relatively constant spinorbit interaction4 within the Pd component of the
Pd/Fe/Pd trili ris, remains constant, then variations in w are dominated by variations
in J. Thus as x decreases toward zero, the increase in J84 gives rise to an increase in
w which in turn gives rise to a more rapid increase in He than would be seen in regular
ferromagnets with constant J. As discussed above, this rapid variation with q ~ 7/3 is
observed experimentally.
The data in Fig. 44 show that T, increases as x increases and reaches a relatively
constant value near x = 20 A. The dashed black line is a guide to the eye and is
qualitatively similar to the behavior of [. !(x) shown in Fig. 42 which saturates at a
larger value near 30 A. These observations are again qualitatively consistent with the finite
size effect associated with critical phenomena in ferrei,, iii, i" ". Although the data are
not of sufficient quality to distinguish the powerlaw behavior that is predicted for finite
size eff. I i183, we expect that the dependence is further complicated by the previously
discussed dependence of J on x in polarized ferromagnetic Pd. The behavior of Tc(x)
Ii, i that Pd/Fe/Pd trili' r should be treated as a single livr with a well defined
spinspin correlation length. If the Pd l zVi~ are treated separately, then the bottom 1 rl.r
CHAPTER 2
DIPOLAR INTERACTIONS AND THEIR INFLUENCE ON THE CRITICAL SINGLE
DOMAIN GRAIN SIZE OF NI IN LAYERED NI/AL20O COMPOSITES
2.1 Abstract
Pulsed laser deposition has been used to fabricate Ni/Al2Os mruiltili, r composites in
which Ni nanoparticles with diameters in the range of 360 nm are embedded as 1l. _i in
an insulating A1203 host. At fixed temperatures, the coercive fields plotted as a function
of particle size show welldefined peaks, which define a critical size that delineates a
crossover from coherently rotating single domain to multiple domain behavior. We observe
a shift in peak position to higher grain size as temperature increases and describe this
shift with theory that takes into account the decreasing influence of dipolar magnetic
interactions from thermally induced random orientations of neighboring grains.
2.2 Introduction
The magnetic properties of nanoparticles have been the focus of many recent
experimental and theoretical studies. Technological improvements have now made it
possible to reproducibly fabricate nanomagnetic particles with precise particle size
and interparticle distances. 1722 These controlled systems have enabled study of the
fundamental properties of single as well as interacting particles. Most applications require
that the particles be single domain with a uniform magnetization that remains stable with
a sufficiently large anisotropy energy to overcome thermal fluctuations,23 which establishes
a temperaturedependent lower bound to the particle size. These considerations must take
into account the effect of interactions on magnetic properties as is evident for highdensity
recording media24 where particles are very close to each other. Considerable insight has
already been gained from experimental studies of the effect of dipolar interaction on
superparamagnetic relaxation time2534 and blocking temperature.29 Less understood
however is the effect of dipolar interactions on the establishment of an upper bound to
particle size, which defines the crossover from single domain (SD) to multi domain (M!l))
behavior. In the following we show using coercivity measurements on Ni/A12Os composites
used phenomenological energy barrier is2,3,47,89
AE =Eo[1 H/Ho] (51)
where Eo is the energy barrier at zero magnetic field and energy barrier vanishes at
H = H0 at T = 0. At H = H,, thermal energy, kBT, is sufficiently high to cause most
of the moments to be thermally activated over the barrier. For example for the case of
StonerWohlfarth particles m = 2, Eo = KV and Ho = 2K/M... For StonerWohlfarth
particles the scenario is very simple and the Eq. 51 can be derived analytically (see
Eq. 16 on page 15 of chapter 1). Remember that if AE(H) is known, it is possible to
calculate H,(T). In this chapter we will discuss how to derive AE(H) (Eq. 51) for the
MD nanoparticles and will compare H,(T) with the model.
5.3 Results and Discussions
The sample preparation technique is discussed in chapter 2 and chapter 3. Three
different sets of samples are investigated. Set 1 consists of single 1ir Ni particles in
an A1203 matrix. Set 2 and Set 3 consists of 5 1. is, of Ni particles separated by A1203
Li,. The interlayer separation in Set 2 and Set 3 are 3 nm and 40 nm respectively. The
schematic of all three sets of samples are shown in Fig. 51 below.
In this chapter we will focus on the temperature dependence of H, for the MD Ni
nanoparticles. A total of 15 samples are studied, 5 samples from each set. Magnetization
loops are measured for every sample for seven (on average) different temperatures. This
means a total of around 105 magnetization loops have been measured for the present
study. Magnetization loops for the sample of average particle diameter of 12 nm of set
2 at different temperatures (indicated in the legends) are shown in Fig. 52. The arrow
shows H, at 10 K. Note that H, decreases with increasing temperature. The temperature
dependence of H, normalized to Ho for five different samples belonging to set 1 is shown
in Fig. 53. The particle diameters are indicated in the legends. Note T2/3 in x axis. All
the data follow a linear T2/3 dependence. To understand the above data, we will start
verifies the absence of the Ni oxide. Samples studied here consists of Ni particle size of 3
nm and 12 nm in diameter.
7.5.2 Gd Thin Film.
Gd thin films were deposited on Si substrates by DC magnetron sputtering. The base
pressure of the chamber was on the order of 5 x 107 Torr. The samples are continuous
with thickness near 100 nm.
7.5.3 (LalyPry)o.67Cao.33MnO3 (LPCMO) Thin Films.
Phase separated manganite (LalyPry)o.67Can, _,u03 (LPC'\O) films were grown
using pulsed laser deposition (PLD) at a rate of 0.05 nm/s on NdGaO3 (NGO) (110)
substrates kept at 820C in an oxygen atmosphere of 420 mTorr11
7.5.4 Temperature Correction of Coercive Field.
For ideal StonerWohlfarth particles the coercive field is given by, Hw = Ho,(T)(1 
(T/TB)1/2). For the case of randomly oriented coherently rotating particles all of which
have the same size, the coercive field is given by, H,"(T) = 0.48H,,(T)(1 (T/TB)3/4).
Since the FePt particles of sample B all have the same size, we can write H,"a(T)
HNH(T) where HNH(T) is the coercive field extracted from the magnetization loops. It is
then straightforward to show that, HW(T) = 2H H(T)(1 (T/TB)/2)(1 (TTB)3/4).
Using the fact that at low fields the zerofieldcooled peak temperature can be identified
as the blocking temperature119, we find that TB = 60 K for the FePt nanoparticles.
Accordingly HSW(T), the abscissa in Fig. 73b, can be calculated in a straightforward
manner from the measured values of TB and H7H(T).
loops measured by a Quantum Design superconducting quantum interference device
(SQUID) after subtracting out the diamagnetic contribution from the substrate. Magnetic
field was applied along the plane of the films. To obtain the magnetization loops, the
magnetic field was varied over the full range (5 T) while keeping temperature fixed.
The high magnetic field data show linear magnetization with magnetic field, which is
due to the diamagnetic contribution from the substrate (as signal from ferromagnetic Ni
particles saturates at high magnetic fields) and can thus be subtracted from the data.
The decrease of H, with increasing temperature for fixed d is clearly apparent and can
be understood as the effect of thermal fluctuations.2 For the lowtemperature isotherms,
there are pronounced peaks which define a temperaturedependent critical particle size
dc delineating SD (d < dc ) behavior of coherently rotating particles from MD (d > d,)
behavior. 2,8,3945 The reason why there is a peak in H,(d) is explained in the introduction
chapter, page 29.
In the inset of Fig. 22 we have plotted H, versus 1/d for the particles of size d > d,
at 10 K. It is clear that H, behaves linearly with 1/d up to particle size of 24 nm and
then saturates. This behavior is consistent with the dependence expected for multidomain
particles. 3 Thus particles of size d > d, are multidomain and the peak defines the
crossover from SD to MD behavior. The formation of domain structure is driven by
the reduction of long range magnetostatic energy, which at equilibrium is balanced by
shorter range exchange and anisotropy energy costs associated with the spin orientations
within a domain wall. The purpose of this chapter is to show that this welldefined SD
region of coherently rotating particles extends over a larger range of grain sizes at higher
temperatures because of the diminishing influence of dipolar interactions from neighboring
grains.
2.4 Data and Discussion
The influence of dipolar interactions on the SD/\!I) crossover can be understood in a
qualitative way by considering the three randomly oriented particles shown schematically
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transition from single domain (SD) to multidomain (M\1)) occurs is given by1 3
36V/A
Rsd = (13)
The above equation is determined by solving the equation Ema, = Ed.13 Thus particles
having radius smaller than Rd are SD and particles having radius larger than Rd are MD
(see Fig. 11).
d < dc d >dc
Figure 11. Smaller (larger) particles are SD (\!1)) as the magnetostatic self energy is
smaller (higher) than the energy required to form domain. The critical size of
the particle where the single domain to multidomain transition occurs is given
by Eq. 13.
The magnetization dynamics for SD and MD particles are dramatically different.
SD particles reverse their magnetization by rotation only. MD particles reverse their
magnetization by domain wall motion and rotation. Rotation of magnetization for the SD
particles is mainly of two types: 1) coherent and 2) incoherent (Fig. 12). The exchange
length24
A (14)
is a measure of the distance over which the atomic exchange interactions dominate and all
the spins rotate coherently. Particles with size larger (smaller) than le rotate incoherently
(coherently). The exchange length is usually larger than Rd for soft ferromagnets where
the anisotropy energy is small. Thus in soft ferromagnets magnetization reversal occurs
either by coherent rotation (small particles) or by domain wall motion (large particles).
BIOGRAPHICAL SKETCH
Ritesh Kumar Das was born on 1981 in a very small village, Mohanbati, located east
of India. At Haripal Guru Dayal high school, Ritesh was introduced to physics and fell in
love with the subject. Ritesh got interested in science subjects during his high school di,
where he found wonderful teachers, Mr. Robin C'i i 1. ijee and Mr. Uttam Saha. After
completing the high school, Ritesh enrolled in the Ramakrishna Mission Vidyamandira
(Belur) in August 1999 and graduated with a Bachelor of Science degree with honors in
physics on August 2002. During this time Ritesh met his favorite teacher Dr. Deepak
Ghsosh, who p1 i, d a very crucial role to make Ritesh interested in experimental physics.
After completing the Bachelor of Science degree, Ritesh enrolled in Master of Science
degree at Indian Institute of Technology (Kanpur) and completed the degree on August
2004. After this Ritesh joined University of Florida to pursue his Ph.D. degree. Ritesh
was ahv, interested in the properties of materials at nanoscale and found that Prof.
A. F. Hebard's lab to be the perfect place for the research in the field of thin films and
nanoparticles. Ritesh graduated in August 2010 with a Doctor of Philosophy degree in
physics.
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be superparamagnetic. For an ideal StonerWohlfarth particle system6 in which all the
particles are aligned along the H direction, a linear square root temperature dependence
of H,(T) is expected. For the considerably more complicated case of randomly oriented
SD particles with a size distribution in which some of the particles are superparamagnetic
(e.g., sample A), H,(T) can be described (solid line of Fig. 71b) using a model with a log
normal size distribution and three fitting parameters9'10 (see Methods). The Hdependent
behavior of AM(H, T) for sample A is shown in Fig. 72a for the temperatures indicated
in the legend. The isotherms show peaks, AMma,(T), at magnetic fields, H,(T), indicated
by the vertical arrows. These peaks are expected, since at H = 0 the FC and ZFC
measurements are equivalent and the difference in magnetization should be zero, whereas
at high H both FC and ZFC magnetizations saturate to the same value and again the
difference should go to zero. The similarities in the AM(H, T) isotherms are ,i'. .1i'.
and become manifest as an unexpected data collapse onto a single curve when the reduced
irreversible magnetization, AM(H, T)/AMmax(T), is plotted as a function of reduced
magnetic field, h(T) = H/H,(T), as done in Fig. 72b. The characteristic field H,(T)
deviates significantly below Hc(T) for T < 25 K (inset of Fig. 72b) and identifies the
Tdependent field where irreversibility is at a maximum.
An important physical insight into the scaling collapse shown in Fig. 72b is gained
by plotting AMmax(T) as a function of T1/2. The observed linear behavior shown in
Fig. 73a is identical to the predicted temperaturedependent coercivity Hs W(T)
of StonerWohlfarth (SW) particles6 mentioned above. Guided by this similarity,
we make the ansatz: AMl a( T) oc H'w. This ansatz is physically reasonable
since as shown above, AM(H, T) measurements are not effected by the presence of
superparamagnetic particles, and in addition the contribution from particles with easy
axis of magnetization along the magnetic field is dominant. As all real samples comprise
particle size distributions and random easy axis orientations, the conventional MH loops
from which coercivities are extracted are markedly different than would occur for idealized
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O 0.4
I
0.2
0.0 .
0 5 10 15 20 25 30 35 40 45 50
T2/3 (K2/3)
Figure 53. Coercive field (He) vs. T2/3 for five different samples of set 1. The linear
behavior is observed for samples with particle size from 18 nm to 42 nm in
diameter.
For the reverse field, ie H 
AE(H)
H the above equation reduces to
(a 4a3(al + boH))3/2
(a 4ala3)3/2
6aj 1
which is in the same form of Eq. 51, where
(a 4ala3)3/2
Eo6a
a 4ala3
4a3bo
From Eq. 57 it is clear that AE(H) decreases with increasing H and when H
energy barrier can be overcome by thermal energy (definition of the coercive field). Thus
H
a 481a3
4a3bo /
(57)
(58)
(59)
He the
respectively along the vertical (H) and perpendicular directions and large enough so that
at the temperature of measurement, changes in magnetization are blocked by energy
barriers that cannot be overcome by thermal activation, and particle 2 (green) with easy
axis along the vertical axis and small enough so that it is superparamagnetic with a
nonhysteretic magnetization depending only on H and T (i.e., unblocked). Consider the
case where only particles 1 and 2 are present. Since the superparamagnetic particle 2 will
have zero AM(H, T), the total AM(H, T) value will be only due to the blocked particle
1. On the other hand, the MH loop will be the summed contributions of the hysteretic
loop for particle 1 and the reversible loop for particle 2 as shown in inset bl of Fig. 7lb.
Thus for this case AM(H, T) is not affected by superparamagnetic particles but He(T)
is. Consider now the case where only particles 1 and 3 are present, i.e., both particles are
blocked but with different (parallel and perpendicular) easy axis orientations with respect
to the applied field. Simple theory for coherently rotating SD particles shows that upon
reversing the field particle 1 must surmount a Hdependent energy barrier whereas particle
3 can line up without having to overcome an energy barrier3. In like manner to the
previous case, The MH loop for particle 1 shows hysteresis but particle 3 does not (inset
b2 of Fig. 71b). Hence H,(T) is affected by the presence of particles with perpendicular
orientation but AM(H, T) is not.
The above arguments can be generalized for SD magnetic nanoparticles with a
broad size distribution and a random orientation of the easy axes of magnetization.
Particles with an easy axis making an arbitrary angle with the applied magnetic field
will alvwb contribute less to hysteresis than aligned particles. Because the perpendicular
component does not contribute, the correction is a straightforward integration over angle.
Accordingly. the measured value of AM(H, T) will be only due to blocked particles and
dominated by particles with easy axis of the magnetization along the applied magnetic
field. On the other hand, H,(T) will be strongly affected by the random orientation of the
easy axis of blocked particles and the presence of the particles which are small enough to
at H = H, the Eq. 57 can be rewritten as
kBT (a
4aia3)3,
6a
H )3/2
H)
ao4ala3
4a360bo
The above equation can be solved for He
H Ho 1 \ ( 2/3
where Hco and Eo are given by Eq. 58 and 59. This temperature dependence of He is
consistent with the experimental results shown in Fig. 53, 54 and 55.
1.0
0.9 Set 2
12 nm
0.8 18 nm
A 24 nm
0.7 v 42 nm
4 60 nm
0 0.6
o 0.5
I
0.4
0.3
0.2
0 5 10 15 20 25 30 35 40 45 50
T2/3 (K2/3)
Figure 54. Coercive field (He) vs. T2/3 for five different samples of set 2. The linear
behavior is observed for samples with particle size from 12 nm to 60 nm in
diameter.
2 (1
(510)
(511)
Abstract of Dissertation Presented to the Graduate School
of the University of Florida in Partial Fulfillment of the
Requirements for the Degree of Doctor of Phil. .. hi,
MAGNETISM IN NANOSCALE MATERIALS, EFFECT OF FINITE SIZE AND
DIPOLAR INTERACTIONS
By
Ritesh Kumar Das
August 2010
C'!I ir: A. F. Hebard
Major: Physics
Material physics is ahv, motivated by the materials with exotic properties. It was
a common belief that exotic properties are only associated with exotic materials. Now
it is clear that geometrical confinement at nanoscale dimensions can give rise to exotic
properties even in simple materials. Ferromagnetic materials in restricted dimensions
are extremely interesting because of their potential applications as well as the rich
fundamental science involved. Magnetic nanoparticles are useful in high density magnetic
data storage devices, sensors, contrast agents in MRI, drug delivery, treating hyperthemia
and many more. All the applications of nanomagnets are very crucial in modern d4v life.
But most of the applications are restricted due to the limitations in the fundamental
properties arises in nanoscale and also due to the technical limitations of controlling things
at nanoscale. For example particles become superparamagnetic as the size is reduced
below a certain value and the magnetization direction fluctuates randomly due to the
thermal energy which limits the density of data storage. The promises of nanomagnets
are huge and to really achieve the grand challenges in nanomagnetism, it is necessary to
understand the basic sciences involve at small scales. In this present work, the magnetic
properties of systems in nanoscale (nanoparticles and thin films) have been investigated.
The effect of dipolar interactions, particle size, particle size distribution, temperature,
magnetic field etc. on the magnetic properties have been studied.
lower the anisotropy energy.
H, H,. (t e) (34)
The "Interaction Field" is a function of the packing fraction (e). Later Wohlfarth51
showed that the effect of the interaction on the He can be increasing or decreasing
depending on the particle orientation as the dipolar interaction is direction dependent.
But all of those results have been constructed considering the fact that the anisotropy
constant, K, either increases or decreases due to the interactions. Previous theoretical and
experimental works have been reported either showing an increase or decrease in H, and
explained in terms of a corresponding increase or decrease in the anisotropy energy.5161,63
In this present experiment we find that an increase in the dipolar interaction increases
H, but decreases de. Equation 31 sil. 1 that the decrease in dc may be due to a
decrease in the K. But a decrease in the K will also decrease r (Eq. 32) and thus will
decrease H, (Eq. 33) which is contradictory to the present experimental result. Thus the
change of K due to the dipolar interactions must not be applicable in the present case. As
any change in K will give rise to change in H, and d, both in the same direction (both
increase or decrease at the same time). Below, we show qualitatively that the increase
in the He can be realized in terms of the collective dynamics of the magnetization of the
particles and decrease in d, can be understood as discussed in reference48
3.3 Results and Discussions
Samples were grown using pulsed laser deposition technique.48 Base pressure of the
growth chamber was on the order of 10' Torr and the growth temperature was around
550" C. Multilayer structure of Al203 and Ni nanoparticle were grown without breaking
the vacuum of the chamber. First a thick (40 nm) buffer livr of Al203 is grown on top
of the substrate. The purpose of this buffer livr is to prevent any diffusion of the Ni into
the substrate. Then Ni nanoparticles and A1203 are sequentially deposited on this buffer
l?vr (see Fig. 1). The top 1v.r of A1203 acts as a capping l,r which prevents oxidation
of the nanoparticles.36 Three different sets of samples are grown. Set 1 and set 2 samples
Now using the expression of E_(H) from Eq. 16 it is easy to show that6
H, Ho [ T 1) (115)
where TB = KV/kBln(Tm/lo) is known as the blocking temperature. Below TB the
anisotropic energy barrier is larger than the thermal energy and magnetization is blocked
or trapped. Above TB the anisotropic energy barrier can be overcome easily by thermal
energy and the particles are called superparamagnetic as will be discussed later. It is clear
from the Eq. 115 that H, decreases with increasing temperature and above the blocking
temperature (T > TB) the particles lose their coercive field. Note that the origin of H,
in a SD particle is the finite time required to reverse the magnetization direction over the
anisotropy energy barrier.
The previous discussion is only true for an assembly of uniform size particles that
have easy axis of magnetization oriented along the same direction with magnetic field
applied along the easy axis. In real samples this is not the case since the easy axis of
magnetization is usually randomly oriented and the particle size is not uniform. A more
general case is shown in Fig. 16 below. Here a arbitrary angle between magnetic field
and the easy axis of magnetization (Q) is considered. The energy of the particle in this
case is7
(1 H
The magnetization of the particle at an applied magnetic field is given by McosO,in,
where O,i, is the angle corresponds to the minima of E(H). Note that here we have
not considered the effect of temperature on the magnetization. At finite temperature
other 0 values around the 0,i, will be occupied with a finite probability according to the
Boltzmann factor as shown in Fig. 17 below. Thus the average over all the occupied
direction with the occupation probability given by the Boltzmann factor will be the
thermal average of the magnetization for a fixed value of H and Q. The procedure should
be repeated for all values of H to get the MH loop for a particular value of Q. Then the
Figure 41.
14.0k
S12.0k
 10.0k
3 8.0k
6.0k
 4.0k
S2.0k
0.0
a) Physical structure
Paramagnetic Pd
Poromngmnetic Pd
Paramagnetic Pd
b) Magnetic structure
a) Multil]i r structure of a Pd/Fe/Pd trilayer. The bottom l ir of Pd is
200 A thick. The thickness of the Fe 1. r is 1.5 A as recorded by the quartz
crystal monitor. The thickness x of the top 1I,r of Pd is varied from 8 to
56 A. b) Magnetic structure of the sample. The total thickness y of polarized
Pd is in the range 20 to 100 A (shaded red area). Thus by varying x, it is
possible to vary the thickness y of the polarized ferromagnetic Pd li. r. c)
Intensity of Fe3 (703.0 eV) LMM Auger electron peak plotted as a function of
material removed by argon sputtering. The data (solid black circles) are fit to
a Gaussian distribution (red line). The full width half maximum value of
1.85 A is consistent with crystal monitor measurements
Auger electron peak of Fig. 41c shows that the Fe is embedded in the Pd as a distinct
2D l ,r with a FWHM thickness of 1.8 A. All of these steps were performed without
breaking vacuum. Measurements of the magnetization M (Fig. 42) were performed
using a Quantum Design MPMS system. The magnetic field H was along the plane of the
substrate. Since the magnetization measurements were ex situ, x was constrained to be
greater than 8 A; otherwise the exposure of the sample to air caused unwanted oxidation
of the Fe. The magnetic parameters H((x) (Fig. 43) and T((x) (Fig. 44) are calculated
respectively from magnetization loops taken at 10 K (see inset of Fig. 43) and linear
extrapolations of the temperaturedependent magnetization taken at H = 20 Oe (see
inset of Fig. 44). The magnetic contribution from the bottom ferromagnetic Pd li, r is
independent of x, since y/2 < 200A, the constant thickness of the bottom 1 VT.
Data
 Gaussian fit
FWHM is i.asA
0 10 20 30 40 50 60
Thickness of the film from the top (A)
c) Auger electron spectroscopy
Equation35 can be rewritten as shown in Eq. 36. Thus the effect of the dipolar
interactions is treated as either an increase (+ Edip) or decrease ( Edip) of anisotropy
energy.
7 0oexp K ) V (3 6)
The effect of dipolar interactions on the He can be explained according to Eq. 36. In
our case a + Edrp increases 7 and give rise to an increase in He with increasing dipolar
interactions (Eq. 32 and 33). If this is to be true in our case then according to Eq. 31,
de should also increase with increasing dipolar interactions. According to the previous
approach both He and de should change in the same way, both increase or both decrease.
In the present experiment we find however that He increases and de decreases due to
dipolar interactions (see Fig. 34) and strongly ii. 1 an alternative approach to the
problem. The effect of dipolar interactions on d, is discussed in reference48, where it
has been shown that the local dipolar magnetic field from the nearby randomly oriented
particles try to align the magnetization direction of the particle in different directions and
thus favoring domain formation. The effect of dipolar interactions on He will be discussed
below in terms of collective dynamics.
It is well known that the magnetization dynamics can be collective in nature due to
the interactions between the particles and the relaxation time (7*) in this case is given
by 64,65
T T > T, (37)
where T is the relaxation time of the single non interacting particle (Eq. 32), T
1 ,, f2/47kBr3 is the critical temperature and depends on the interparticle distance
and particle magnetization and z is a critical exponent. The above equation clearly
i I i that the relaxation time will be larger in the presence of dipolar interactions
and thus according to Eq. 33 He will be larger, and thus agreeing with our experimental
smooth substrate independent starting surface for the growth of Fe, as verified by high
resolution scanning transmission electron microscopy studies (Fig. 21). A 40 nmthick
cap 1. r of A1203 was deposited to protect the Fe 1vr from oxidation. Three different
samples with thickness of 9 nm, 21 nm and 30 nm were prepared for the present study.
Magnetization measurements are performed in a quantum design Magnetic Property
Measurement System (\!PMS). The magnetic field was along the plane of the films. The
dependence of temperature and film thickness on coercive field is investigated.
6.4 Results and Discussion
4.0x10 O M10K
m M50K
2.0x10 M100K
? M150K /
E 0M.0
5 2.0x10 M250K
M300K
4.0x104 M325
6.0x10 0
8.0x1 0 
600 400 200 0 200 400 600
H (Oe)
Figure 62. MH loop of Fe film of thickness 21 nm at different temperatures as indicated
in the legend. The coercive field defined at M=0, decreases with increasing
temperature.
Shown in Fig. 61 is the TEM image of the 9 nm thick Fe sample. Due to the
low surface energy difference between Fe and A1203 (650 mJ/m2) and high adhesion
energy (1205 mJ/m2) between Fe and Al203,100 Fe wets the surface of Al203 and thus
a continuous thin film is grown instead of grains as is the case for the Ni/AO203 system
discussed in chapter 2 and 3. Three different samples with thickness 9 nm, 21 nm and
30 nm were grown. The magnetic hysteresis loops at different temperatures from 10 K
to 350 K are measured with the applied magnetic field along the plane of the thin film.
MH loops for 21 nm sample are shown in Fig. 62. The magnetic field is swept from 5
200 
/ 3
180 % Mvs T(x = 56A)at200e
2
U E
0 T ............
140 c
i 100 200 300
T(K)
0 20 40 60
x (A)
Figure 44. The Curie temperature T, rapidly increases with increasing x. Data are shown
as solid black circles and the dashed black line is a guide to the ev.
Saturation to a constant value occurs near 20A (vertical arrow) The inset with
T, indicated by the vertical arrow shows the temperaturedependent
magnetization taken in a field H = 20 Oe.
where B8 is the Brillouin function and p is the number of the nearest neighbors beyond
which J is zero. In principle the experimentally determined values of M(H, T, x) can be
fit to Eq. 41 to find the best fit values of J(x) for different values of the parameter p. We
have not performed such an ,in !1i
Fig. 43 shows the behavior of the coercivity H,(x) as a function of x (solid black
circles). The data are well described by a powerlaw dependence (solid black line),
H,(x) oc x", where the exponent r = 2.3(0.1) is close to the ratio 7/3. Similar
powerlaw behavior reveals itself in regular ferromagnetic thin films where q has a
somewhat smaller value varying from 0.3 to 1.576. Because rl depends strongly on strain,
roughness, impurity, and the nature of the domain wall (Bloch or Neel type)76, it is not
surprising to see a wide variation in Tl. Neel predicted for example that for Bloch domain
walls, He of a ferromagnetic thin film should vary as x4/3 when the thickness x of the film
4.4 Results and Discussion .................. ........ .. .. 54
4.5 Conclusions .................. ................ .. 58
5 TEMPERATURE DEPENDENCE OF COERCIVITY IN MULTI DOMAIN
NI NANOPARTICLES, EVIDENCE OF STRONG DOMAIN WALL PINNING 59
5.1 Abstract ...................... ............. 59
5.2 Introduction ...................... ........... 59
5.3 Results and Discussions ............................ 60
5.4 Relation Between Micromagnetic Parameter and Magnetic Parameters 65
5.5 Conclusions ...................... ........... 66
6 COERCIVE FIELD OF FE THIN FILMS AS THE FUNCTION OF TEMPERATURE
AND FILM THICKNESS: EVIDENCE OF NEEL DISPERSE FIELD THEORY
OF MAGNETIC DOMAINS ................... ....... 68
6.1 Abstract ...................... ............. 68
6.2 Introduction ...................... ........... 68
6.3 Experimental Details ................... ....... 69
6.4 Results and Discussion ................... ...... 70
6.5 Conclusion ...................... ........... 74
7 SCALING COLLAPSE OF THE IRREVERSIBLE MAGNETIZATION OF
FERROMAGNETIC THIN FILMS ............. ........... 75
7.1 Abstract ....................... ............ 75
7.2 Introduction ...................... ........... 75
7.3 Experimental Results .................. ........... .. 76
7.4 Conclusions .................. ................ .. 84
7.5 Methods ................... ............... 85
7.5.1 Ni N i'" .q. iticle. .................. .......... .. 85
7.5.2 Gd Thin Film. .. ..... .. .......... 86
7.5.3 (Lai_yPry)0.67Ca,, M!O3 (LPC'1O) Thin Films. ... 86
7.5.4 Temperature Correction of Coercive Field. ..... 86
REFERENCES ................... ............. ...... 87
BIOGRAPHICAL SKETCH ........... ........ ... 96
8.0xl104 
4
6.0x104 
4.0x104 
2.0x104 
0.0
2.0x104 
4.0x104 
6.0x104 
8.0x104 
e
500 1000 1500
H (Oe)
Figure 52. Magnetization loops for the sample of average particle diameter of 12 nm of
set 2 at different temperatures (indicated in the legends). The coercive field
(He) at 10 K is indicated by the arrow. He decreases with increasing
temperature. Saturation magnetization (3[.,) is constant at different
temperatures.
The two solutions for the above equations are
a2 + 4/3(aj boH)
2a3
a2 V 4a3(a bo0H)
(54)
(55)
Taking the second derivative of E(x) with respect to x it is easy to show that
62E/6X2 Ix,> 0 (62E/6X2 IX2< 0) and corresponds to the maximum (minimum). Thus the
energy barrier is
(a2 4ala3 + 4a3boH)3/2
AE(H) = E(xi) E(x2) a
6a3
o MsublOK
 Msub50K
MsublOOK
 Msubl50K
 Msub200K
 Msub250K
 Msub300K
 Msub325K
24 nm Ni/AIl20
5 Layer
l)
11111J11
1500 1000 500
__
(56)
where dw/dx can be thought of as the resistance of the domain wall motion. In real
samples due to the impurities, imperfections, strains etc, dW/dx passes through
maxima and minima. The wall motion over these maxima and minima is irreversible
in magnetic field and that is the origin of the hysteresis. The coercive field, the measure of
irreversibility, is usually given by2'11
1
H = (dW/dx)Tmax
211. 9
There are different theoretical models to calculate (dW/dx),ax for different imperfections
in the sample and the results for some of them are listed in Tablel1.
Table 11. Table here lists some known models along with the variation of coercive field
according to the model.
Theory He System References
StonerWohlfarth H = 2K [1 (kBg I /KV)1/2] SD, CR nanoparticle with uniaxial
StonerWohlfarth
Micromagnetic
Inclusion Theory
Inclusion Theory
Inclusion Theory
Inclusion Theory
Inclusion Theory
H, = [1 ( Ig
H = (kB
H, 2K
Ms
S/KV)3/4]
r 2/3
2/3
Hc =
M,/d
H,  1/2(ln2L)
H, ( )3/2,
H 2 = [0.386 + log 2 ]
H, = 3ylo/Md2
anisotropy along the applied magnetic field
SD, CR nanoparticle with uniaxial
anisotropy randomly oriented
MD, 2 phase material, hard magnet, a3 is
the micromagnetic parameter and depends
on the K, Ms, A
MD system, d < 6, free pole energy is
ignored, coercivity is assumed to be equal
to the maximum pining field, d is the
diameter of the inclusion, 6 is the domain
wall thickness, 7 is the domain wall energy
per unit area, a is the volume fraction of
the inclusion
MD system, d > 6, free pole energy is
ignored, L is the linear dimension of the
sample
MD system, d < 6, free pole energy is ig
nored
MD system, d < 6, free pole energy is con
sidered
MD system, closer domain, large inclusion,
commonly seen in the case of Neel's spike, I
is the equilibrium length of the spike
1.4 Magnetization vs. Temperature
Until now we have been discussing the behavior of magnetization as a function of
magnetic field at a fixed temperature. Now we will discuss how magnetization changes
with the temperature at a fixed magnetic field. At small applied magnetic field, spins
are trapped in metastable energy minima separated by energy barriers from the global
(121)
7
12
11,13
11,14
11,14
15
16
consist of 5 1l ri of Ni nanoparticles separated by A12O3 1V, r. For set 1 (set 2) the
A1203 separation is 3 nm (40 nm). Set 3 samples are single l1vr of Ni nanoparticles in
A1203 matrix. Dipolar interactions are strongest in set 1, moderate in set 2 and weakest
in set 3. The dipolar interactions are stronger in Set 1 compared to set 2 as the interlayer
separation of the Ni particles is smaller in set 1 compared to set 2. Set 3 consists of only
a single 1 v, of Ni particles and thus the dipolar interactions are weakest. All sets of
samples consist of different samples with varying particle size from 3 nm to 60 nm.
C) 1 41 1 1 4 4 4
Estate
Multi Layer
Figure 31.
Fig la) shows the TEM image of a single 1i,r sample with average particle
diameter of ~ 24 nm. Particles are well defined with inter particle distance of
around 4 nm. Ib) shows a schematic of the single lv, r sample. A 40 nm thick
buffer 1v,.r of A1203 is first grown on top of substrate. Then the Ni
nanoparticles are grown on to of the buffer 1V.r. Finally a 3 nm thick capping
lIv,r of A12O3 is grown to protect it from oxidation. ic) shows the schematic
of 5 liv.i~ of Ni nanoparticle sample.
Figure 3la) shows the TEM image of the single lv, r Ni particles with average
particle diameter of ~ 24 nm (set 3). The simplified schematic of the single and rmiltil ivr
samples are shown in 31 b) and c).
Typical magnetization loops at three different temperatures are shown in Fig.
32a) for the sample with 3 nm A1203 spacer lv1 r (set 1) and 6 nm in diameter. The
coercive field H,(T) is determined from the loop as shown by the arrow. This procedure
to determine H, is repeated for all samples belonging to all three sets. At temperatures
a)
b) 4 44
statee
Single Layer
CHAPTER 5
TEMPERATURE DEPENDENCE OF COERCIVITY IN MULTI DOMAIN NI
NANOPARTICLES, EVIDENCE OF STRONG DOMAIN WALL PINNING
5.1 Abstract
The temperature dependence of the coercivity of the single and 5 liv r samples of
Ni nanoparticles in A1203 matrix is studied. A linear T2/3 dependence of coercivity over
a wide range of temperature (10 K to 350 K) is observed. All the samples consists of
particles with multiple magnetic domains as the size of the particles are larger than the
critical single domain size (see Eq. 13 on page 13 of chapter 1 and Fig. 33 on page 47
of chapter 3). The experimental results are understood in terms of strong domain wall
pinning.
5.2 Introduction
The temperature dependence of the extrinsic magnetic properties, for example
coercive field (H,(T)), arise from two mechanisms. The first mechanism is, due to
the temperature dependence of the intrinsic magnetic properties 11,15'86'7 such as
saturation magnetization (. [.), magnetic anisotropy (K) and exchange stiffness (A)
and will be discussed in chapter 6. The second mechanism is, due to the thermally
activated hoping of the metastable states over some energy barrier.24,6 From the
magnetization loops at different temperatures (Fig. 52) we have found that [., does
not change with temperature. All the samples comprise pcl i, i I l 11iiw. par !I. and
thus magne' i, 1 iii.w anisotropy can be neglected and temperature independent shape
anisotropy is dominant.48 The experimental temperature range is 10 K to 300 K which is
much smaller than the curie temperature of Ni (630 K)3 and A can be considered constant
over this temperature range."8 In this chapter we will discuss the second mechanism as the
origin of the temperature dependence of the coercive field (11.,, K and A are temperature
independent). To understand the temperature dependence of the He due to the thermally
activated hopping over metastable energy minima separated by some energy barrier, it is
necessary to find out the magnetic field dependence of the energy barrier. A commonly
4
2
E
2
4
6E5
1500 1000 500 0 500 1000 1500
H (Oe)
Figure 19. Hysteresis loop of a Single 1~v. r Ni nanoparticles of 18 nm diameter embedded
in an Al203 matrix at temperature, T < TB. The loops show well defined
coercive field (where magnetization is zero) and decreases with increasing
temperatures.
superparamagnet). The magnetization for a collection of superparamagnetic particles is
given by the Langevin equation
MsVH kBT
M(H, T) V N .V[coth M] (117)
kBT 11.,VH
where N is the number of particles. Note that M is a function of H/T in the above Eq.
117. Thus if M is plotted as the function of H/T for different T, all the MH loops will
fall on top of each other as shown in Fig. 110 for a single l v.r sample of 12 nm Ni grains
in an A1203 host matrix.
1.3 Hysteresis Loop of Multi Domain Particles
In multidomain ferromagnetic system the origin of the hysteresis loop is dramatically
different than the SD case. Usually in soft ferromagnets (Rsd < le) the SD and MD
particles can be distinguished by the behavior of the coercive field as a function of
particle size. Figure 111 below is a schematic showing the behavior of coercive field as a
* 10 K
. 50 K ====
100 K **."u,,:
* 150K U/n i U
200 K = ,
,,,," 
/ U/
U
200' K E
15 M10K
10 M50K
M100K, /
0
5
5
10 H,
15
1.5 1.0 0.5 0.0 0.5 1.0 1.5
H (KOe)
b)
10
5
0
S5
S10
a)
E
L
Figure 32. a) Magnetization loop of a sample from set 1 of average particle diameter of ~
6nm. Coercive field (H,) is determined from the loop as shown by the arrow.
H, decreases with increasing temperature and goes to zero above the blocking
temperature. b) Magnetization loops above blocking temperatures.
Magnetization is plotted as the function of H/T to show the
superparamagnetic behavior as expected for the SD particles above the
blocking temperature.
above the blocking temperatures (TB) SD samples behave as superparamagnetic particles.
Figure 32b) shows the superparamagnetic behavior of the set 1, 6 nm diameter sample.
Note the magnetization data fall on top of each other when plotted as a function of H/T.
This behavior is a direct consequence of the superparamagnetic behavior as expected from
the coherently rotating SD particles.
Figure 33 shows H, plotted as a function of d for the set 1, set 2 and set 3 samples.
The data that correspond to the different sample sets are indicated in the legends. The
peak in the He separates SD and MD particles. 2,8,41,42,44,48 It is clear from the data that
dc decreases with increasing dipolar interactions (de1 < d,2 < d). H, on the other hand
increases with the increasing dipolar interactions (vertical dotted arrow) in the SD region.
These two results can not be explained in terms of the commonly reported change in K
due to the dipolar interactions.5161 The decrease in d, due to the dipolar interactions has
been discussed elsewhere.48 In this present study, the collective dynamics of the particles
6 4 2 0 2 4 6
H/T(Oe/K)
M250K
o M300K
M325K
' J ,
and/or impurities in the material107. For the simplest case of single domain coherently
rotating nanoparticles, the origin of hysteresis is the finite time scale for magnetization
reversal as the magnetization overcomes a magnetic field dependent energy barrier by
thermal activation and rotates from one easy axis direction to another5'6'106. Hysteresis
and associated magnetization reversals p1 i, an important role in applications such as
magnetic data storage devices91 93, GMR94'95 or MRAM96 devices, magnetic , i i.'' and
motors98, generators99 etc.
7.3 Experimental Results
Measurements of irreversible magnetization are usually accomplished by one or both
of two techniques illustrated respectively in panels a) and b) of Fig. 71. The sample
under investigation in this figure (hereafter referred to a sample A) is a 20 Athick pulsed
laser deposited thin film comprising five l~V iS of 3 nm elongated Ni particles embedded
in an insulating Al203 host [see Methods]. The Ni particles are small enough to be in the
single domain (SD) regime where all the spins are aligned in the same direction and rotate
coherently together in response to a changing magnetic field. In the first technique (panel
a), the sample is field cooled (FC) in a field H = 20 Oe (black squares) from 300 K to 5 K
and then zero field cooled (ZFC). The irreversible magnetization (AM(H, T)), which is a
function of magnetic field (H) and temperature (T), is shown by the twoheaded dashed
vertical arrow. In the second technique, the sample is held at fixed temperature T and
magnetization M loops obtained by repeatedly cycling the applied field H about H = 0
between two symmetric limits. The history dependent trajectories form closed loops shown
schematically in the insets of panel (b). These loops, which can be acquired at different
temperatures, are each characterized by a coercive field H,(T), a saturated moment .[.,(T)
and a remnant magnetization Mr(T). The coercive field H,(T), plotted versus T1/2 in
panel b for sample A discussed above, is shown as a blue line connecting the starred data
points. The absence of a T1/2 dependence for coherently rotating SD particles with easy
axes oriented along the field6 will be discussed below. While both AM(H, T) and H,(T)
Figure 21. Cross sectional dark field STEM image of a 51i r NiAl203 sample grown on
caxis sapphire
experiment the grain size d, as measured by the amount of Ni deposited referenced to a
calibrated standard, represents the average size of the diskshaped grains shown in the
figure. This calibration was obtained from crosssectional TEM micrographs of single l1.r
 i1 !1. '' by comparing the average grain size with d. The TEM observation also shows
that the Al203 spacer l.ri~ are partially crystallized. Due to the large surface energy
difference between Ni and A1203 Ni forms welldefined, separated islands within the
Al203 matrix.36 Previous studies on similarlyprepared samples using atomic number (Z)
contrast imaging in TEM together with electron energy loss spectroscopy (EELS) have
confirmed the absence of NiO at the Ni/A1203 interfaces.36 The Ni/A1203 interfaces were
chemically abrupt without an intermixing between Ni, Al and oxygen. In addition we did
not observe exchangebias induced .*,mmetric magnetization loops, thus lending support
to the conclusions of previous studies36 that antiferromagnetic NiO is absent in our 1 ,, i, t
Ni/A1203 system.
Previous TEM studies on single lir samples have shown the particles to be
p&I, *1 ,1 ilii,. For example, a three nm particle comprising three crystalline grains
.In the absence of interactions (Hd = 0) the condition for the SD to MD transition
is given for spherical particles with radius d/2 by, Ad = Bd2 where Ad' is the total
magnetostatic energy and Ed, = Bdc is the domain wall energy.46 We have absorbed
the factor of two, which relates diameter to radius, into the constants A and B In the
presence of the dipolar magnetic field Hd the formation of domain walls will be assisted
by a Zeeman term which is proportional to the volume of the affected particle. The
condition determining the SD to MD transition now becomes,
Ad = Bd 7ri.. .,1'/6 (24)
When the dipolar interaction is a small perturbation, i.e., 3 [f,/A < 1, Eq. 21 and
24 can be combined to give the relation,
(1 e()
dc = dco ddw 3( (25)
V/7P(erfi(3) erfi(vP 1 ))
where dco = B/A is the temperatureindependent critical diameter in the absence of
interactions (hightemperature limit) and dd, = poBM2Tr/(72A2) for a = r/3. The second
term on the righthand side of Eq. 25 thus becomes a temperaturedependent correction
to dc due to interactions from neighboring particles and decreases with increasing T .
Since the magnetic field due to the dipoledipole interactions are weaker at higher
temperatures Eq. 21, the nanoparticles remain in the SD state to a larger size, which
by Eq. 25 results in a shift of dc towards higher values at higher temperatures. This is
indeed evident in Fig. 23, which shows the temperature dependence of dc as determined
from the data in Fig. 22. The black squares are the simulated data according to Eq. 25
using the two fitting parameters: dco and dd, Qualitatively, the data agree quite well
with the prediction of the theoretical model without taking into account the topology
and size distribution of the particles. We have found dco = 84 nm from our simulation
(Fig. 23, black squares) to be close to the value for a particle with shape anisotropy
constant Kshape = 3.1 x 104 J3 (do = 72AeK/,,,JV where Ae, is exchange stiffness,
CHAPTER 4
FINITE SIZE EFFECTS WITH VARIABLE RANGE EXCHANGE COUPLING IN
THINFILM PD/FE/PD TRILAYERS
4.1 Abstract
The magnetic properties of thinfilm Pd/Fe/Pd trilayers in which an embedded
~1.5Athick ultra thin 1. r of Fe induces ferromagnetism in the surrounding Pd have
been investigated. The thickness of the ferromagnetic trilayer is controlled by varying
the thickness of the top Pd 1v,r over a range from 8 A to 56 A. As the thickness of the
top Pd 1 r decreases, or equivalently as the embedded Fe 1, r moves closer to the
top surface, the saturated magnetization normalized to area and the Curie temperature
decrease whereas the coercivity increases. These thicknessdependent observations for
proximitypolarized thinfilm Pd are qualitatively consistent with finite size effects that
are well known for regular thinfilm ferromagnets. The functional forms for the thickness
dependence, which are strongly modified by the nonuniform exchange interaction in
the polarized Pd, provide important new insights to understanding nanomagnetism in
twodimensions.
4.2 Introduction
The presence of 3d magnetic transition metal ions in palladium (Pd) gives rise to
giant moments thus significantly enhancing the net magnetization 6670. Pd is known to
be in the verge of ferromagnetism because of its strong exchange enhancement with a
Stoner enhancement factor of ~ 1071. The magnetic impurities induce small moments on
nearby Pd host atoms thereby creating a cloud of polarization with an associated giant
moment71'72. Neutron scattering experiments show that the cloud of induced moments can
include ~200 host atoms with a spatial extent in the range 10 to 50 A72,73. Thus a thin
1I, of Fe encapsulated within Pd will be sandwiched between two ..11i i'.ent thin l,' is of
ferromagnetic Pd with nonuniform magnetization and a total thickness in the range 20 to
100 A.
4.5E5
M275K
3 M300K
E2 M325K
0
2
'3 At
4.5E5
3 2 1 0 1 2 3
H/T(Oe/K)
Figure 110. Hysteresis loop of a SD coherently rotating particle at temperature (T > TB).
Sample shows zero coercive field as expected for superparamagnetic particles.
Note the H/T abscissa. Magnetization is plotted as a function of H/T for
three different temperatures as indicated in the legend. Loops at all different
temperatures fall on top of each other as predicted by the Langevin equation
for superparamagnetic particles.
function of particle size. For very small particles the coercive field is zero and particles are
superparamagnetic (SP) with magnetization determined by the Langevin function. As the
particle size is increased, the coercive field increases due to the fact that the energy barrier
increases. Particles with size larger than the critical single domain radius are multidomain
and the coercive field decreases with increasing particle size.2,3,9 This may be due to the
fact that as particle size increases the number of domains increases and thus it is easier to
have domain closure which decreases coercivity because there is less total magnetization.
The size dependence of the coercivity in MD region is experimentally found to be2
HcMD = a + b/d" (118)
where a, b are constants that depend on the real structure factor and materials, d is the
diameter of the particles and x has value around 1.2 There is no theoretical model that

Full Text 
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MAGNETISMINNANOSCALEMATERIALS,EFFECTOFFINITESIZEANDDIPOLARINTERACTIONSByRITESHKUMARDASADISSERTATIONPRESENTEDTOTHEGRADUATESCHOOLOFTHEUNIVERSITYOFFLORIDAINPARTIALFULFILLMENTOFTHEREQUIREMENTSFORTHEDEGREEOFDOCTOROFPHILOSOPHYUNIVERSITYOFFLORIDA2010 1
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c2010RiteshKumarDas 2
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Idedicatethistomyparentsandfamilyfortheiractivesupport.Withoutthemitwouldhavenotbeenpossible. 3
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ACKNOWLEDGMENTS Iamtrulyindebtedtomanyindividualswhohavecontributedtothesuccessofmyresearchwork.Therefore,Iexpressmysincerestregretstoanypersonnotspecicallymentionedhere.Firstandforemost,IamthankfultomyresearchadvisorProf.A.F.Hebardforgivingmetheopportunitytoworkwithhim.Ithasbeenagreatexperiencetoworkunderhissupervision.Hispositive,openmindedattitudetowardresearchcreatesauniquelaboratoryenvironmentfullofencouragement.Ihavelearnedalotfromhisunadulteratedenthusiasm,willingnesstolearnandelegantbutsimpleapproachtounderstandingfundamentalphysics.Iwouldliketothankallthepresentandformerlabmembersfortheirhelpsandpleasantcompany.IamgratefultoJohnJ.KellyforteachingmemanyexperimentaltechniqueswhenIjoinedthegroup.ThankstoallthelabmembersPatrick,Rajiv,Sef,Siddhartha,Sanal,Xiaochangfortheirhelps.Ireallyenjoyedworkingwithyouguys.Iwouldalsoliketoacknowledgethestasofmachineshopandelectricshop.Speciallycryogenicstas,GregandJohn,fortheirconstantsupplyofliquidHeandN2allyeararound24/7.ThankstoJay(reallyaniceguy)forlookingafterallthepumpsandchillers.Iwouldliketothankallofmycommitteemembers.IwillspeciallythanksProf.AmlanBiswas.ThoughIdidnothavechancetocollaboratewithhim,buthisguidanceandsupporttowardsmydegreehavebeenveryhelpful.IamalsogreatlythankfultoProf.D.Nortonforthewonderfulcollaborationandforlettingmeusehislabfacilities.IamthankfultomycollaboratorsD.KumarandA.GuptafromNCA&T.IamalsoverythankfultoMatt,Patrick,KyeongWonfromProf.Norton'slabfortheirhelpsandbeinggoodfriends. 4
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Iamindebtedtomyparentsfortheirsupport,encouragementandforalwaysbelievinginme.IappreciatethewarmthandaectionofmysisterMridula.Icouldnothavecomethisfarwithouttheirblessings. 5
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TABLEOFCONTENTS page ACKNOWLEDGMENTS ................................. 4 LISTOFTABLES ..................................... 8 LISTOFFIGURES .................................... 9 ABSTRACT ........................................ 11 CHAPTER 1THEORYANDBACKGROUND .......................... 12 1.1SingleDomainandMultiDomainParticles .................. 12 1.2HysteresisLoopofSingleDomainCoherentlyRotatingParticles ...... 14 1.3HysteresisLoopofMultiDomainParticles .................. 24 1.4Magnetizationvs.Temperature ........................ 29 1.4.1ZeroFieldCooled(ZFC)Magnetization ................ 30 1.4.2FieldCooled(FC)Magnetization ................... 31 2DIPOLARINTERACTIONSANDTHEIRINFLUENCEONTHECRITICALSINGLEDOMAINGRAINSIZEOFNIINLAYEREDNi/Al2O3COMPOSITES 32 2.1Abstract ..................................... 32 2.2Introduction ................................... 32 2.3ExperimentalDetails .............................. 33 2.4DataandDiscussion .............................. 36 2.5Conclusion .................................... 40 2.6Methods ..................................... 41 2.6.1MathematicalAnalysis ......................... 41 2.6.2BasicPhysicalUnderstanding ..................... 41 3EFFECTOFDIPOLARINTERACTIONONTHECOERCIVEFIELDOFMAGNETICNANOPARTICLES:EVIDENCEFORCOLLECTIVEDYNAMICS 42 3.1Abstract ..................................... 42 3.2Introduction ................................... 42 3.3ResultsandDiscussions ............................ 44 3.4Conclusions ................................... 49 4FINITESIZEEFFECTSWITHVARIABLERANGEEXCHANGECOUPLINGINTHINFILMPd/Fe/PdTRILAYERS ...................... 51 4.1Abstract ..................................... 51 4.2Introduction ................................... 51 4.3ExperimentalDetails .............................. 52 6
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4.4ResultsandDiscussion ............................. 54 4.5Conclusions ................................... 58 5TEMPERATUREDEPENDENCEOFCOERCIVITYINMULTIDOMAINNINANOPARTICLES,EVIDENCEOFSTRONGDOMAINWALLPINNING 59 5.1Abstract ..................................... 59 5.2Introduction ................................... 59 5.3ResultsandDiscussions ............................ 60 5.4RelationBetweenMicromagneticParameterandMagneticParameters .. 65 5.5Conclusions ................................... 66 6COERCIVEFIELDOFFETHINFILMSASTHEFUNCTIONOFTEMPERATUREANDFILMTHICKNESS:EVIDENCEOFNEELDISPERSEFIELDTHEORYOFMAGNETICDOMAINS ............................. 68 6.1Abstract ..................................... 68 6.2Introduction ................................... 68 6.3ExperimentalDetails .............................. 69 6.4ResultsandDiscussion ............................. 70 6.5Conclusion .................................... 74 7SCALINGCOLLAPSEOFTHEIRREVERSIBLEMAGNETIZATIONOFFERROMAGNETICTHINFILMS ......................... 75 7.1Abstract ..................................... 75 7.2Introduction ................................... 75 7.3ExperimentalResults .............................. 76 7.4Conclusions ................................... 84 7.5Methods ..................................... 85 7.5.1NiNanoparticle. ............................. 85 7.5.2GdThinFilm. .............................. 86 7.5.3(La1)]TJ /F5 7.97 Tf 6.59 0 Td[(yPry)0:67Ca0:33MnO3(LPCMO)ThinFilms. .......... 86 7.5.4TemperatureCorrectionofCoerciveField. .............. 86 REFERENCES ....................................... 87 BIOGRAPHICALSKETCH ................................ 96 7
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LISTOFTABLES Table page 11Hcvs.T ........................................ 29 8
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LISTOFFIGURES Figure page 11SDandMDparticle ................................. 13 12Coherentandincoherentrotation .......................... 14 13Singleparticleinmagneticeld ........................... 15 14Twostateenergy ................................... 16 15HysteresisofSDparticle ............................... 18 16Diagramofaparticle ................................. 20 17Thermalaverageofmagnetization .......................... 21 18Flowdiagram ..................................... 21 19MHbelowTB ..................................... 24 110MHbelowTB ..................................... 25 111SDtoMDtransitionandHc ............................. 26 112MagnetizationloopforMDparticle ......................... 27 113DomainwallandHc ................................. 28 114Mvs.Tfor3nmNinanoparticles ......................... 30 21STEMimageofNiparticle .............................. 34 22Hcvs.d,dierentT ................................. 35 23dcvs.T ........................................ 37 24Hdanddomain .................................... 41 31Sample ......................................... 45 32MHloop ........................................ 46 33Hcvs.d:dipolarinteraction ............................. 47 34Dipolarinteraction .................................. 49 41Physicalandmagneticviewofsample ....................... 53 42Saturationmagnetizationvs.x ........................... 54 43Coerciveeldvs.x .................................. 55 9
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44Curietemperaturevs.x ............................... 56 51Threesetsofsample ................................. 61 52MHloopsofset2 ................................... 62 53Hcvs.T2=3set1samples .............................. 63 54Hcvs.T2=3set2samples .............................. 64 55Hcvs.T2=3set3samples .............................. 65 56Hc0andE0ofset2 .................................. 66 61TEMimageofFelm ................................ 69 62MHloopofFelm .................................. 70 63Hcvs.TofFelm .................................. 71 64Hcvs.KofFelm .................................. 72 65Hcvs.dofFelm .................................. 74 71IrreversibleMagnetization .............................. 77 72BehavioroftheM(H;T)isothermsasthefunctionofHandscalingcollapse 80 73Theanstz ....................................... 81 74Scalingcollapseofvarietyofferromagneticmaterials ............... 83 10
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AbstractofDissertationPresentedtotheGraduateSchooloftheUniversityofFloridainPartialFulllmentoftheRequirementsfortheDegreeofDoctorofPhilosophyMAGNETISMINNANOSCALEMATERIALS,EFFECTOFFINITESIZEANDDIPOLARINTERACTIONSByRiteshKumarDasAugust2010Chair:A.F.HebardMajor:Physics Materialphysicsisalwaysmotivatedbythematerialswithexoticproperties.Itwasacommonbeliefthatexoticpropertiesareonlyassociatedwithexoticmaterials.Nowitisclearthatgeometricalconnementatnanoscaledimensionscangiverisetoexoticpropertieseveninsimplematerials.Ferromagneticmaterialsinrestricteddimensionsareextremelyinterestingbecauseoftheirpotentialapplicationsaswellastherichfundamentalscienceinvolved.Magneticnanoparticlesareusefulinhighdensitymagneticdatastoragedevices,sensors,contrastagentsinMRI,drugdelivery,treatinghyperthemiaandmanymore.Alltheapplicationsofnanomagnetsareverycrucialinmoderndaylife.Butmostoftheapplicationsarerestrictedduetothelimitationsinthefundamentalpropertiesarisesinnanoscaleandalsoduetothetechnicallimitationsofcontrollingthingsatnanoscale.Forexampleparticlesbecomesuperparamagneticasthesizeisreducedbelowacertainvalueandthemagnetizationdirectionuctuatesrandomlyduetothethermalenergywhichlimitsthedensityofdatastorage.Thepromisesofnanomagnetsarehugeandtoreallyachievethegrandchallengesinnanomagnetism,itisnecessarytounderstandthebasicsciencesinvolveatsmallscales.Inthispresentwork,themagneticpropertiesofsystemsinnanoscale(nanoparticlesandthinlms)havebeeninvestigated.Theeectofdipolarinteractions,particlesize,particlesizedistribution,temperature,magneticeldetc.onthemagneticpropertieshavebeenstudied. 11
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CHAPTER1THEORYANDBACKGROUND Ferromagnetismisknownformorethan2500yearstoman.Therstmagneticmaterialdiscoveredwasmagnetite(Fe2O3).Thepracticalapplicationsofferromagnetswasrecognizedfromveryancienttime.Therstuseofmagneticmaterialwasasacompass.Accordingtothemagneticproperties,materialscanbedividedintodiamagnetic,paramagnetic,ferromagnetic,antiferromagnetic,ferrimagnetic,spinglassetc.Inthispresentworkferromagnetismwillbethemaintopic.Chaptersfollowedbythischapterwilldiscusstheeectofnitesizeanddipolarinteractionsonthemagneticpropertiesofsomematerialswithnanoscalestructures.Inthischapterageneraltheoreticalbackgroundwillbegiven. 1.1SingleDomainandMultiDomainParticles Whenthesizeoftheparticleisverysmall,itwillcontainonlyonemagneticdomain. 1 { 3 Thisisbecausetheenergyrequiredtoformadomainislargerthanthemagnetostaticselfenergy.Themagnetostaticselfenergyforasphericalparticleisgivenby 1 Emag=0M2sV=12(1{1) where0isthefreespacepermeability,MsisthesaturationmagnetizationandVisthevolumeoftheparticle.TheenergyrequiredtoformaBlochdomainwallis 1 { 3 Edw=4p AKR2(1{2) whereKistheanisotropyconstant,AistheexchangestinessandRistheradiusoftheparticle. NotethatEmaggrowsasR3andEdwgrowsasR2.Domainformationisthereforefavorableforlargerparticlesasthemagnetostaticenergywillbelargecomparedtothedomainwallformationenergy.Thecriticalsingledomainradius(Rsd)wherethe 12
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transitionfromsingledomain(SD)tomultidomain(MD)occursisgivenby 1 { 3 Rsd=36p AK 0M2s(1{3) TheaboveequationisdeterminedbysolvingtheequationEmag=Edw. 1 { 3 ThusparticleshavingradiussmallerthanRsdareSDandparticleshavingradiuslargerthanRsdareMD(seeFig. 11 ). Figure11. Smaller(larger)particlesareSD(MD)asthemagnetostaticselfenergyissmaller(higher)thantheenergyrequiredtoformdomain.ThecriticalsizeoftheparticlewherethesingledomaintomultidomaintransitionoccursisgivenbyEq. 1{3 ThemagnetizationdynamicsforSDandMDparticlesaredramaticallydierent.SDparticlesreversetheirmagnetizationbyrotationonly.MDparticlesreversetheirmagnetizationbydomainwallmotionandrotation.RotationofmagnetizationfortheSDparticlesismainlyoftwotypes:1)coherentand2)incoherent(Fig. 12 ).Theexchangelength 2 { 4 lex=s A 0M2s(1{4) isameasureofthedistanceoverwhichtheatomicexchangeinteractionsdominateandallthespinsrotatecoherently.Particleswithsizelarger(smaller)thanlexrotateincoherently(coherently).TheexchangelengthisusuallylargerthanRsdforsoftferromagnetswheretheanisotropyenergyissmall.Thusinsoftferromagnetsmagnetizationreversaloccurseitherbycoherentrotation(smallparticles)orbydomainwallmotion(largeparticles). 13
PAGE 14
Figure12. Coherentandincoherentrotationofthemagnetization.Incaseofcoherentrotationallthespinsrotatetogetherandthewholeparticlecanbeconsideredasagiantspin.CoherentrotationhappensforSDparticleswithsizesmallerthantheexchangelengthlex 1.2HysteresisLoopofSingleDomainCoherentlyRotatingParticles ThemagnetizationdynamicsoftheSDparticleswithR
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Figure13. ASDparticleinanappliedmagnetic(H)eldalongtheeasyaxisofmagnetization(k).istheanglebetweenthemagnetizationMandtheeasyaxisk. oftheenergyoccursat==2separatingthetwoenergyminima.Figure 14 a)showstheenergydiagramatzeromagneticeldasafunctionof.Inthiscasetheparticlewillhavemagnetizationparalleltotheeasyaxisofmagnetizationsincethesecorrespondtominimumenergystates(upordown).Anyotherdirectionswillcostsomeanisotropyenergy.ThetwostateswithminimumenergyareseparatedbytheanisotropyenergybarrierequaltoKV.InanappliedmagneticeldalongtheeasyaxisthetwoenergyminimawillbeshiftedduetotheZeemanenergy(Fig. 14 b)).NowthestatealongthemagneticeldwillbemoststableastheenergyisloweredduetotheZeemanterm.Thestatewithoppositedirectionofmagnetizationwillbemetastable.Themagneticelddependentenergybarrierforthespinup(E+(H))anddown(E)]TJ /F1 11.955 Tf 7.08 1.79 Td[((H))stateiscalculatedbyStonerandWohlfarthtobe, 6 E(H)=KV1H Hco2(1{6) whereE+(H)istheenergybarrierseenbytheupmagnetizedparticlesandE)]TJ /F1 11.955 Tf 7.09 1.8 Td[((H)istheenergybarrierseenbythedownmagnetizedparticlesandHc0=2K=Ms.DerivationoftheEq. 1{6 isgivenbelow. 15
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Figure14. TwostateenergyofaSDparticle.Twoenergyminimacorrespondtothedirectionoftheeasyaxisofmagnetization.a)Atzeromagneticeldtheparticlewillhavemagnetizationalongtheeasyaxisofmagnetizationasthosecorrespondtominimumenergystates(upanddown).UpanddownstatesareseparatedbytheenergybarrierequaltoKV.Toreversethemagnetizationdirectionfromuptodownorviceversathesystemhastoovercometheenergybarrier. 5 BrownproposedthatthisprocessrequiresanitetimegivenbyEq. 1{14 5 b)Inanappliedmagneticeldalongtheeasyaxis,thetwoenergyminimawillbeshiftedduetotheZeemanenergy.Nowtheupstatewhichisalongtheappliedmagneticeldwillbemoststableandhavethelowestenergy.Thestatewithoppositedirection(downstate)ofmagnetizationwillbemetastable.ThemagneticelddependentenergybarrierforthespindownstateiscalculatedbyStonerWohlfarth(Eq. 1{6 ) 6 FirstorderderivativeofEq. 1{5 withrespecttois E(H) =2KVsincos+MsVHsin(1{7) Atthemaximaandminima 2KVsincos+MsVHsin=0(1{8) Solutionsoftheaboveequationare sin=0(1{9) cos=)]TJ /F6 11.955 Tf 10.5 8.09 Td[(MsH 2K(1{10) 16
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TakingthesecondorderderivativeofEq. 1{5 ,itcanbeshownthattheEq. 1{9 (Eq. 1{10 )referstominima(maximum)oftheenergy.Thustheenergyminimaareat=0and=andmaximumatwhencos=MsH=2K(seeFig. 14 ).Energiescorrespondtotheseextremaare Emin+=)]TJ /F6 11.955 Tf 9.3 0 Td[(MsVH (1{11) Emin)]TJ /F1 11.955 Tf 16.71 2.87 Td[(=MsVH (1{12) Emax=KV"1+MsH 2K2# (1{13) whereEmin+andEmin)]TJ /F1 11.955 Tf 10.66 2.87 Td[(correspondsto=0(spinup)and=(spindown)respectively.ItisnoweasytoshowthatE+(H)=EmaxEmin+andE)]TJ /F1 11.955 Tf 7.09 1.8 Td[((H)=EmaxEmin)]TJ /F1 11.955 Tf 10.66 2.87 Td[(aregivenbyEq. 1{6 Theenergybarrierhastobeovercometoreversethemagnetizationdirectionfromuptodownorviceversa.Brownproposedthatthisprocessrequiresanitetime 5 =0expE(H) kBT(1{14) whereTisthetemperature,)]TJ /F3 7.97 Tf 6.58 0 Td[(10istheinverseattemptfrequencyofovercomingtheenergybarrierandkBistheBoltzmannconstant. Figure 15 showsthemagnetizationprocesswhenthemagneticeldissweptfromalargepositivevaluetoalargenegativevalueandagainfromanegativetopositivevaluetocompletethemagnetizationloop.Whenmagneticeldislarge(scenario1)allparticleswillbemagnetizedalongthemagneticeldandapositivesaturationmagnetizationisachieved.Asmagneticeldisreducedtozero(scenario2)themagnetizationdirectionwillbetrappedintheupdirectionasthetemperatureisnotenoughtoovercometheenergybarrier.Nowasthemagneticeldisreversedtheenergybarrier,E)]TJ /F1 11.955 Tf 7.09 1.8 Td[((H)willbereducedaccordingtoEq. 1{6 (scenario3).Butstillthetemperatureisnotenoughtoovercometheenergybarrierandthemagnetizationwillstillbetrappedwithapositivevalue.Afurtherincreaseinmagneticeldintheoppositedirectionwillkeeploweringtheenergy 17
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barrieruntil,atthecoerciveeld,theenergybarriercanbeovercomebythethermalenergyandmagnetizationreversalwilloccur(scenario4).WhenH=Hctheenergy Figure15. HysteresisofacoherentlyrotatingSDparticle.Scenario1)Highpositivemagneticeldisappliedandsaturationmagnetizationisobserved.Scenario2)Magneticeldisreducedfrompositivevaluetozero.Magnetizationistrappedinthepositivedirectionasthethermalenergyisnotenoughtoovercometheenergybarrier.Scenario3)Magneticelddirectionisreversed.Stilltheenergybarrierislargecomparedtothethermalenergyandmagnetizationistrappedinthepositivedirection.Scenario4)Magneticeldequalstothecoerciveeld.Nowtheenergybarriercanbeovercomebythermalenergyandmagnetizationreversaloccurs. barrierE)]TJ /F1 11.955 Tf 7.09 1.79 Td[((Hc)issuchthattherelaxationtime)]TJ /F1 11.955 Tf 10.99 1.79 Td[(=matthetemperatureT.Wheremistheexperimentalmeasurementtime(around100secforSQUIDmeasurement).ThuswhenH=Hc,magnetizationreversaloccurs.CombiningEq. 1{6 and 1{14 ,thecoercivity(Hc(T))oftheSDparticlecanbecalculatedasshownbelow. )]TJ /F1 11.955 Tf 17.05 1.79 Td[(=m=0expE)]TJ /F1 11.955 Tf 7.08 1.79 Td[((Hc) kBT)E)]TJ /F1 11.955 Tf 7.09 1.79 Td[((Hc)=kBTlnm 0 18
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NowusingtheexpressionofE)]TJ /F1 11.955 Tf 7.09 1.79 Td[((H)fromEq. 1{6 itiseasytoshowthat 6 Hc=Hc0"1)]TJ /F8 11.955 Tf 11.96 16.86 Td[(T TB1 2#(1{15) whereTB=KV=kBln(m=0)isknownastheblockingtemperature.BelowTBtheanisotropicenergybarrierislargerthanthethermalenergyandmagnetizationisblockedortrapped.AboveTBtheanisotropicenergybarriercanbeovercomeeasilybythermalenergyandtheparticlesarecalledsuperparamagneticaswillbediscussedlater.ItisclearfromtheEq. 1{15 thatHcdecreaseswithincreasingtemperatureandabovetheblockingtemperature(T>TB)theparticleslosetheircoerciveeld.NotethattheoriginofHcinaSDparticleisthenitetimerequiredtoreversethemagnetizationdirectionovertheanisotropyenergybarrier. Thepreviousdiscussionisonlytrueforanassemblyofuniformsizeparticlesthathaveeasyaxisofmagnetizationorientedalongthesamedirectionwithmagneticeldappliedalongtheeasyaxis.Inrealsamplesthisisnotthecasesincetheeasyaxisofmagnetizationisusuallyrandomlyorientedandtheparticlesizeisnotuniform.AmoregeneralcaseisshowninFig. 16 below.Hereaarbitraryanglebetweenmagneticeldandtheeasyaxisofmagnetization( )isconsidered.Theenergyoftheparticleinthiscaseis 7 E(H)=2KV1 2sin2( )]TJ /F6 11.955 Tf 11.95 0 Td[())]TJ /F6 11.955 Tf 16.89 8.09 Td[(H Hc0cos(1{16) ThemagnetizationoftheparticleatanappliedmagneticeldisgivenbyMcosmin,whereministheanglecorrespondstotheminimaofE(H).Notethatherewehavenotconsideredtheeectoftemperatureonthemagnetization.AtnitetemperatureothervaluesaroundtheminwillbeoccupiedwithaniteprobabilityaccordingtotheBoltzmannfactorasshowninFig. 17 below.ThustheaverageoveralltheoccupieddirectionwiththeoccupationprobabilitygivenbytheBoltzmannfactorwillbethethermalaverageofthemagnetizationforaxedvalueofHand .TheprocedureshouldberepeatedforallvaluesofHtogettheMHloopforaparticularvalueof .Thenthe 19
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Figure16. Singleparticleinanappliedmagneticeld(H).kisthedirectionoftheeasyaxisofmagnetization.MandHarethemagnetizationandmagneticeldvectorsrespectively.WithoutloosinganygeneralityMandHcanbeconsideredinthesameplane.TheanglebetweenMandHis.TheanglebetweenHandkis .TheenergybarrierforthisgeneralcongurationisgivenbyEq. 1{16 7 MHloopsforallpossible shouldbecalculated.AveragingoveralltheseMHloopswillgiveamagnetizationloopattemperatureTforasampleofuniformparticlesizeandarandomlyorientedeasyaxisofmagnetization.Alltheaboveproceduresshouldbedoneforallpossibleparticlesizesastherealsamplesusuallyhavesomeparticlesizedistribution.Theprobabilityofaparticularparticlesizecanbemodeledeitherasalognormalorgaussiandistributionfunction.Inthiswaythemagnetizationloopofarealsamplewithnonuniformparticlesizeandrandomorientationoftheeasyaxisofmagnetizationcanbedetermined.Ifthealltheaboveproceduresarerepeatedfordierenttemperaturesthenthemagnetizationloopatdierenttemperaturescanbedetermined.Belowweshowaowdiagramfortheaboveprocess. 7 { 9 20
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Figure17. AtnitetemperatureothervaluesaroundminwillbeoccupiedwithaniteprobabilityaccordingtotheBoltzmannfactorandshownbytheshadedregion.Thethermalaverageofthemagnetizationwillbetheaverageoftheallmagnetizationdirectionsoverthisshadedregion. 7 TheprobabilityofhavingsomemagnetizationdirectionwillbedeterminedbytheBoltzmannfactor. 1 Startwiththeenergyofthesingleparticle. E(H)=2KV1 2sin2( )]TJ /F6 11.955 Tf 11.96 0 Td[())]TJ /F5 7.97 Tf 16.59 4.7 Td[(H Hc0cos + 2 FindtheminimaofE(H) MsVCosminwillbethemagnetizationatT=0forthegivenvalueofH, andV Figure18. Flowdiagramtoshowtheprocessofcalculatingcoerciveeldforrealnanoparticlesampleswithparticlesizedistributionandrandomorientationoftheeasyaxisofmagnetizationsatnitetemperature. 21
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+ 3 Thermalaverageofthemagnetization hM(H; ;V)iT=R21MsVcosexp)]TJ /F11 5.978 Tf 8.92 2.35 Td[(E kBTd R21exp)]TJ /F11 5.978 Tf 8.92 2.34 Td[(E kBTd E=E)]TJ /F6 11.955 Tf 11.96 0 Td[(Emin1and2areshowninFig. 17 hM(H; ;V)iTisthemagnetizationattemperature=TforthegivenvalueofH, andV + 4 Step1,2and3shouldberepeatedfordierentH.ThiswilldeterminetheMHloopforagivenvalueofT, andV + 5 Step1,2,3and4shouldberepeatedforallpossible andaverageofallthoseloopswilldeterminetheMHloopforagivenvalueofTandVforanensembleofparticleswithrandomorientationoftheeasyaxisofmagnetization. + Figure18. continued 22
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6 Step1,2,3,4and5shouldberepeatedfordierentparticlesizetodeterminetheMHloopforagivenvalueofTforasampleconsistingofnonuniformparticlesizeandrandomorientationoftheeasyaxisofmagnetization.Inrealsamplestheparticledistributionfunctionisusuallylognormalorgaussian. 9 10 + 7 Step1,2,3,4,5and6shouldberepeatedfordierentTtodeterminethetemperaturedependenceoftheMHloop. 7 + 8 Completionofstep7willprovideanopportunitytodeterminethetemperaturedependenceofthecoerciveeld,remanentmagnetizationetc.SomeofthetemperaturedependentofcoerciveeldsarelistedinTable 11 Figure18. continued MagnetizationloopsatdierenttemperaturesforasinglelayersampleofNinanoparticlesofaveragediameteraround18nmareshowninFig. 19 .Thecoerciveeldisdeterminedbythemagneticeldwheremagnetizationchangessignandpassesthroughzero.ItisclearfromtheFig. 19 thatcoerciveeldsdecreaseswithincreasingtemperatureasdiscussedabove.AttemperatureshighcomparedtotheanisotropyenergyKV,themagnetizationdirectionscanrotatefreelyoverthebarrierandtheparticlesbecomesuperparamagneticwithHc=0.InthiscasethesystemcanbetreatedsimilartothecaseofparamagnetismwitheachparticleasagiantorsuperspinofvalueMsV(thuscalled 23
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Figure19. HysteresisloopofaSinglelayerNinanoparticlesof18nmdiameterembeddedinanAl2O3matrixattemperature,T
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Figure110. HysteresisloopofaSDcoherentlyrotatingparticleattemperature(T>TB).Sampleshowszerocoerciveeldasexpectedforsuperparamagneticparticles.NotetheH=Tabscissa.MagnetizationisplottedasafunctionofH=Tforthreedierenttemperaturesasindicatedinthelegend.LoopsatalldierenttemperaturesfallontopofeachotheraspredictedbytheLangevinequationforsuperparamagneticparticles. functionofparticlesize.Forverysmallparticlesthecoerciveeldiszeroandparticlesaresuperparamagnetic(SP)withmagnetizationdeterminedbytheLangevinfunction.Astheparticlesizeisincreased,thecoerciveeldincreasesduetothefactthattheenergybarrierincreases.Particleswithsizelargerthanthecriticalsingledomainradiusaremultidomainandthecoerciveelddecreaseswithincreasingparticlesize. 2 3 9 Thismaybeduetothefactthatasparticlesizeincreasesthenumberofdomainsincreasesandthusitiseasiertohavedomainclosurewhichdecreasescoercivitybecausethereislesstotalmagnetization. ThesizedependenceofthecoercivityinMDregionisexperimentallyfoundtobe 2 HcMD=a+b=dx(1{18) wherea,bareconstantsthatdependontherealstructurefactorandmaterials,disthediameteroftheparticlesandxhasvaluearound1. 2 Thereisnotheoreticalmodelthat 25
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Figure111. Coerciveeldplottedasafunctionofparticlediameter.Forverysmallparticlesthecoerciveeldiszeroandtheparticlesareknownassuperparamagneticparticles(SP).Astheparticlesizeisincreasedthecoerciveeldincreasesduetothefactthattheenergybarrierincreases.Particleswithsizelargerthanthecriticalsingledomainradiusaremultidomainandcoerciveelddecreaseswithincreasingparticlesize. explainsthebehaviorinEq. 1{18 .ThusthethepeakinthecoerciveeldwhenplottedasthefunctionoftheparticlesizedelineatestheSDandMDbehavior.InexperimentwehavefoundthesamebehaviorforbothmultilayerandsinglelayersamplesofNiparticlesinAl2O3matrixaswillbediscussedindetailinchapter 2 Figure 112 showsthepossibledomainwallcongurationfordierentpointsinthemagnetizationloop.RememberthatcomparedtotheSDcasewheretheoriginofthehysteresiswasthehoppingoveraenergybarrier,incaseofMDtheoriginofhysteresisisirreversibledomainwallmotion.Atveryhighmagneticeldallthespinsinthesystemwillbealignedalongthemagneticeldandpositivesaturation(Ms)willbeachieved(Fig. 112 ).Asthemagneticeldisreducedtozeroadomainwallwillbeformed.Duetotheimperfectionsinthesample,thedomainwallwillbestuckinapositionsuchthattheupdomainislargerthanthedowndomainandnetmagnetizationorremanent 26
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magnetization(Mr)willbeseenatzeromagneticeld.Reversingthemagneticeldwill Figure112. HysteresisloopofaMDsystemandpossibledomainwallconguration.Atverylargepositivemagneticeldallthespinsarealignedalongthemagneticeldandsaturationmagnetizationisachieved.Whenmagneticeldisreducedtozero,adomainwallforms.Duetotheimperfectionsinthesample,thedomainwallwillbestuckinapositionsuchthattheupdomainislargerthanthedowndomainandremanentmagnetizationismeasured.Ifthedirectionofthemagneticeldisreversedthedomainwallwillstarttomovetotherightandthedowndomainwillgrow.Atamagneticeldequaltothecoerciveeld,thedownandupdomainwillbeequalinsizeandmagnetizationwillbezero.Foralargenegativemagneticeldthedomainwallbemovedtotherightandallthespinswillbeinthedirectionofthemagneticeldandnegativesaturationwillbereached. movethedomainwalltotherightsideandthusthedowndomainwillstarttogrowandmagnetizationwillbereduced.Whenthenegativemagneticeldisequalstothecoerciveeldtheupanddowndomainwillhavesamesizeandmagnetizationwillbezero.Furtherincreaseinmagneticeldinthenegativedirectionwillforcethedomainwalltomoveallthewaytorightmakingallspinsalignedalongthemagneticeldandnegativesaturationwillbereached. 27
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ToderivethecoerciveeldinMDdomaincaseconsiderasimplecase,asshowninFig. 113 ,whereasingledomainwallseparatestwodomains.Therighthandsideisaspinupdomainandlefthandsideisaspindowndomain.Inanappliedmagneticeld,H, Figure113. Singledomainwallseparatingtwomagneticdomains.Righthandsideisaspinupdomainandlefthandsideisaspindowndomain.InanappliedmagneticeldduetotheZeemanenergythedomainwallwillexperienceapressureandsomeworkneedtobedonetomovethewallagainstthispressure.TheoriginofhysteresisinMDsampleistheirreversiblemotionofthedomainwall. alongthespinupdomain,theZeemanenergyoftheup(down)domainwillbe)]TJ /F6 11.955 Tf 9.3 0 Td[(MsH(+MsH)perunitvolume.Thustheenergydierenceacrossthedomainwallwillbe)]TJ /F1 11.955 Tf 9.3 0 Td[(2HMSperunitvolume.Thisenergydierencecanbeconsideredasapressureonthewallandsomeworkhastobedonetomovethedomainwallagainstthispressure.Theworkdonetomovethewalladistancedxis 2 11 dW=2MsHSdx(1{19) whereStheareaofthedomainwall.Thustheworkdonetomovethewallbyunitdistanceis 2 11 dW=dx=2MsHS(1{20) 28
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wheredw=dxcanbethoughtofastheresistanceofthedomainwallmotion.Inrealsamplesduetotheimpurities,imperfections,strainsetc,dW=dxpassesthroughmaximaandminima.Thewallmotionoverthesemaximaandminimaisirreversibleinmagneticeldandthatistheoriginofthehysteresis.Thecoerciveeld,themeasureofirreversibility,isusuallygivenby 2 11 Hc=1 2MsS(dW=dx)max(1{21) Therearedierenttheoreticalmodelstocalculate(dW=dx)maxfordierentimperfectionsinthesampleandtheresultsforsomeofthemarelistedinTable 11 Table11. Tableherelistssomeknownmodelsalongwiththevariationofcoerciveeldaccordingtothemodel. TheoryHc SystemReferences StonerWohlfarthHc=2K Ms[1)]TJ /F11 5.978 Tf 7.45 0 Td[((kBTlnm 0=KV)1=2] SD,CRnanoparticlewithuniaxialanisotropyalongtheappliedmagneticeld 2 6 StonerWohlfarthHc=0:96K Ms[1)]TJ /F11 5.978 Tf 7.45 0 Td[((kBTlnm 0=KV)3=4] SD,CRnanoparticlewithuniaxialanisotropyrandomlyoriented 7 MicromagneticHc=2K Ms)]TJ /F11 5.978 Tf 7.45 0 Td[([3p ja3j 4kBTlnm 0]2=3 MD,2phasematerial,hardmagnet,a3isthemicromagneticparameteranddependsontheK,Ms,A 12 InclusionTheoryHc=2=3 Msd MDsystem,d<,freepoleenergyisignored,coercivityisassumedtobeequaltothemaximumpiningeld,disthediameteroftheinclusion,isthedomainwallthickness,isthedomainwallenergyperunitarea,isthevolumefractionoftheinclusion 11 13 InclusionTheoryHc=1:751=2 MsL(ln2L d) MDsystem,d>,freepoleenergyisignored,Listhelineardimensionofthesample 11 14 InclusionTheoryHc=2:81=2 MsL(d )3=2(ln2L ) MDsystem,d<,freepoleenergyisignored 11 14 InclusionTheoryHc=2K Ms[0.386+logr 2M2s K] MDsystem,d<,freepoleenergyisconsidered 15 InclusionTheoryHc=3l=Msd2 MDsystem,closerdomain,largeinclusion,commonlyseeninthecaseofNeel'sspike,listheequilibriumlengthofthespike 16 1.4Magnetizationvs.Temperature Untilnowwehavebeendiscussingthebehaviorofmagnetizationasafunctionofmagneticeldataxedtemperature.Nowwewilldiscusshowmagnetizationchangeswiththetemperatureataxedmagneticeld.Atsmallappliedmagneticeld,spinsaretrappedinmetastableenergyminimaseparatedbyenergybarriersfromtheglobal 29
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minima.Asthetemperatureisincreasedthespinscanhopovertheenergybarriertoreachtheglobalminima.Duetothistrappingofspinsinlocalminima,magnetizationvaluesdependsstronglyonthecoolingprotocol.Therearemainlytwodierentcoolingprotocols,eldcooled(FC)andzeroeldcooled(ZFC).ThebehaviorofmagnetizationasafunctionoftemperatureforthetwoprotocolsisshowninFig. 114 belowforthesampleofNinanoparticlesof3nmdiameteratanappliedeldof20Oe.ThetemperaturewherethedierencebetweenFCandZFCdisappearsisgenerallycalledtheirreversibletemperature(Tirr).FornanoparticlesTirrissameastheblockingtemperature(TB). 2 Figure114. Magnetizationvs.temperatureatanappliedmagneticeldof20Oeforthe3nmdiameterNinanoparticles.Theredcoloristheeldcooled(FC)magnetizationandtheblackoneisthezeroeldcooled(ZFC)magnetization. 1.4.1ZeroFieldCooled(ZFC)Magnetization Zeroeldcooledmagnetizationismeasuredbycoolingthesamplefromhightemperature(temperatureabovetheirreversibletemperature(Tirr))withoutanyappliedmagneticeld.Atlowtemperatureasmallmagneticeldisappliedandmagnetizationismeasuredasafunctionoftemperatureduringthewarmupwhilekeepingthemagneticeldon.HerewewilldiscusstheshapeoftheZFCmagnetizationinaqualitativemanner.Ingeneralthemagneticsystemcanbetreatedasatwostateproblemasshownpreviously 30
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inFig. 14 wherespinupanddowncorrespondtotheenergyminimaseparatedbysomeenergybarrier.TheoriginoftheenergybarrierintheSDcaseistheanisotropywhereasforthecaseofMDtheoriginisdomainwallpinningatdefects.Athightemperaturetheenergybarrieriseasilyovercomeduetothethermalenergyandthespinupanddownstateswillbeequallypopulated.ThusathightemperatureaboveTirr,magnetizationwillbezero.Nowifthesampleiscooledtoalowtemperaturewithoutanyappliedmagneticeld,thenzeromagnetizationstatewillbeblockedastheenergybarrierisnowlargecomparedtothethermalenergy. 2 3 6 Ifasmallmagneticeldisappliedthechangeinmagnetizationwilloccuronlyforthesmallenergybarriersthatcanbeovercomeatthattemperatureandasmallmagnetizationwillbeachieved.Astemperatureisincreased,theprobabilityofovercomingthelargerbarriersincreasesandmagnetizationincreases.AttemperatureTirrtheprobabilitiestoovercomethebarrierforspinupanddownbecomenearlyequalandthespinupanddownmixingstartstohappenandthusmagnetizationdecreaseswithfurtherincreaseintemperature. 1.4.2FieldCooled(FC)Magnetization Fieldcooledmagnetizationismeasuredbycoolingthesamplefromhightemperaturetothelowtemperatureinanappliedmagneticeldandmagnetizationismeasuredduringthewarmupprocess. 2 Inthiscaseathightemperatureduetotheappliedmagneticeld,thespinupstatesaremorepopulatedthanthespindownstates.Coolingthesampleatalowtemperaturewhilekeepingtheeldonwillthuslockthesysteminmagnetizedstate.Anincreaseintemperaturewillincreasetheprobabilityofspinupanddownmixingandthusmagnetizationwillgraduallydecrease. 31
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CHAPTER2DIPOLARINTERACTIONSANDTHEIRINFLUENCEONTHECRITICALSINGLEDOMAINGRAINSIZEOFNIINLAYEREDNI/AL2O3COMPOSITES 2.1Abstract PulsedlaserdepositionhasbeenusedtofabricateNi/Al2O3multilayercompositesinwhichNinanoparticleswithdiametersintherangeof360nmareembeddedaslayersinaninsulatingAl2O3host.Atxedtemperatures,thecoerciveeldsplottedasafunctionofparticlesizeshowwelldenedpeaks,whichdeneacriticalsizethatdelineatesacrossoverfromcoherentlyrotatingsingledomaintomultipledomainbehavior.Weobserveashiftinpeakpositiontohighergrainsizeastemperatureincreasesanddescribethisshiftwiththeorythattakesintoaccountthedecreasinginuenceofdipolarmagneticinteractionsfromthermallyinducedrandomorientationsofneighboringgrains. 2.2Introduction Themagneticpropertiesofnanoparticleshavebeenthefocusofmanyrecentexperimentalandtheoreticalstudies.Technologicalimprovementshavenowmadeitpossibletoreproduciblyfabricatenanomagneticparticleswithpreciseparticlesizeandinterparticledistances. 17 { 22 Thesecontrolledsystemshaveenabledstudyofthefundamentalpropertiesofsingleaswellasinteractingparticles.Mostapplicationsrequirethattheparticlesbesingledomainwithauniformmagnetizationthatremainsstablewithasucientlylargeanisotropyenergytoovercomethermaluctuations, 23 whichestablishesatemperaturedependentlowerboundtotheparticlesize.Theseconsiderationsmusttakeintoaccounttheeectofinteractionsonmagneticpropertiesasisevidentforhighdensityrecordingmedia 24 whereparticlesareveryclosetoeachother.Considerableinsighthasalreadybeengainedfromexperimentalstudiesoftheeectofdipolarinteractiononsuperparamagneticrelaxationtime 25 { 34 andblockingtemperature. 29 Lessunderstoodhoweveristheeectofdipolarinteractionsontheestablishmentofanupperboundtoparticlesize,whichdenesthecrossoverfromsingledomain(SD)tomultidomain(MD)behavior.InthefollowingweshowusingcoercivitymeasurementsonNi/Al2O3composites 32
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thatwithincreasingtemperaturethisupperboundtoparticlesizeincreasesandthensaturatesduetoattenuateddipolarinteractionsfromthermallyinducedcoherentmotionsofthemagnetizationoftheneighboringrandomlyorientedparticles. 2.3ExperimentalDetails ThecompositesystemstudiedinthispapercompriseselongatedandpolycrystallineNiparticleswithdiametersintherangeof360nmembeddedaslayersinaninsulatingAl2O3host.ThemultilayersampleswerefabricatedonSi(100)orsapphire(caxis)substratesusingpulsedlaserdepositionfromaluminaandnickeltargets.HighpuritytargetsofNi(99.99%)andAl2O3(99.99%)werealternatelyablatedfordeposition.Beforedeposition,thesubstrateswereultrasonicallydegreasedandcleanedinacetoneandmethanoleachfor10minandthenetchedina49%hydrouoricacid(HF)solutiontoremovethesurfacesilicondioxidelayer,thusforminghydrogenterminatedsurfaces. 35 Thebasepressureforallthedepositionswasoftheorderof10)]TJ /F3 7.97 Tf 6.59 0 Td[(7Torr.Aftersubstrateheating,thepressureincreasedtothe10)]TJ /F3 7.97 Tf 6.59 0 Td[(6Torrrange.Thesubstratetemperaturewaskeptatabout550oCduringgrowthoftheAl2O3andNilayers.Therepetitionrateofthelaserbeamwas10Hzandenergydensityusedwas2Jcm)]TJ /F3 7.97 Tf 6.59 0 Td[(2overaspotsize4mm1.5mm.A40nmthickbuerlayerofAl2O3wasdepositedinitiallyontheSiorsapphiresubstratebeforethesequentialgrowthofNiandAl2O3.ThisprocedureresultsinaverysmoothstartingsurfaceforgrowthofNiasveriedbyhighresolutionscanningtransmissionelectronmicroscopystudies(Fig. 21 ).Multilayersampleswerepreparedhaving5layersofNinanoparticlesspacedfromeachotherby3nmthickAl2O3layers.A3nmthickcaplayerofAl2O3wasdepositedtoprotectthetopmostlayerofNinanoparticles. ShowninFig. 21 isacrosssectionalTEMimagefromamultilayered(5layers)NiAl2O3samplegrownoncplanesapphire.TheNiparticleshaveasizeof235nminwidthand9nminheight.Theseparationbetweenneighboringparticlesisontheorderof3nm(measuredasaprojecteddistanceincrosssectionalview),whichiscomparabletothethicknessoftheAl2O3spacerlayers.Forthepurposesofthis 33
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Figure21. CrosssectionaldarkeldSTEMimageofa5layerNiAl2O3samplegrownoncaxissapphire experimentthegrainsized,asmeasuredbytheamountofNidepositedreferencedtoacalibratedstandard,representstheaveragesizeofthediskshapedgrainsshowninthegure.ThiscalibrationwasobtainedfromcrosssectionalTEMmicrographsofsinglelayersamples 36 bycomparingtheaveragegrainsizewithd.TheTEMobservationalsoshowsthattheAl2O3spacerlayersarepartiallycrystallized.DuetothelargesurfaceenergydierencebetweenNiandAl2O3,Niformswelldened,separatedislandswithintheAl2O3matrix. 36 Previousstudiesonsimilarlypreparedsamplesusingatomicnumber(Z)contrastimaginginTEMtogetherwithelectronenergylossspectroscopy(EELS)haveconrmedtheabsenceofNiOattheNi/Al2O3interfaces. 36 TheNi/Al2O3interfaceswerechemicallyabruptwithoutanintermixingbetweenNi,Alandoxygen.Inadditionwedidnotobserveexchangebiasinducedasymmetricmagnetizationloops,thuslendingsupporttotheconclusionsofpreviousstudies 36 thatantiferromagneticNiOisabsentinourlayeredNi/Al2O3system. PreviousTEMstudiesonsinglelayersampleshaveshowntheparticlestobepolycrystalline.Forexample,athreenmparticlecomprisingthreecrystallinegrains 34
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hasbeenobserved. 36 Polycrystallineparticleswillthereforehavecrystallinegrainsorientedindierentdirections,thustendingtoaverageanynetcrystallineanisotropytozero.Accordingly,temperatureindependentshapeanisotropyisdominantandtemperaturedependentcrystallineanisotropycanbeneglected.Inaddition,itisalsoimportanttonotethattheexchangelengthlex=14.6nmforNi, 37 whichisthelengthscalebelowwhichatomicexchangeinteractionsdominateovermagnetostaticelds,determinesthecriticalradii(Rcoh)forcoherentrotation:Rcoh5lexforsphericalparticlesandRcoh3:5lexfornanowires. 3 Theparticlesizes(1.530nminradius)thatwehaveinvestigatedarethussmallerthanthecriticalradiusbelowwhichcoherentrotationofNiprevails. Figure22. Coercivityfor5layerNi/Al2O3multilayersamples(5repeatedunits)plottedasafunctionofparticlesize(diameter)atthetemperaturesindicatedinthelegend.Thepeakpositionsatd=dcforeachisotherm,indicatedbyverticalarrows,delineatethecrossoverfromsingledomain(SD)tomultipledomain(MD)behavior(d>dc).InsetshowsthebehaviorofHcasafunctionof1=dfortheparticleswithd>dcat10K.Thelineardependenceupto24nmdiameterparticleswithsaturationataconstantvalueforlargeparticles 38 isconsistentwiththebehaviorexpectedformultidomainparticles.Thusparticlesontherighthandsideofthepeakaremultidomain. InFig. 22 weshowplotsofHcasafunctionofparticlesizedateachofthetemperaturesindicatedinthelegend.Coerciveeldswereextractedfrommagnetization 35
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loopsmeasuredbyaQuantumDesignsuperconductingquantuminterferencedevice(SQUID)aftersubtractingoutthediamagneticcontributionfromthesubstrate.Magneticeldwasappliedalongtheplaneofthelms.Toobtainthemagnetizationloops,themagneticeldwasvariedoverthefullrange(5T)whilekeepingtemperaturexed.Thehighmagneticelddatashowlinearmagnetizationwithmagneticeld,whichisduetothediamagneticcontributionfromthesubstrate(assignalfromferromagneticNiparticlessaturatesathighmagneticelds)andcanthusbesubtractedfromthedata.ThedecreaseofHcwithincreasingtemperatureforxeddisclearlyapparentandcanbeunderstoodastheeectofthermaluctuations. 2 Forthelowtemperatureisotherms,therearepronouncedpeakswhichdeneatemperaturedependentcriticalparticlesizedcdelineatingSD(ddc)behavior. 2 8 39 { 45 ThereasonwhythereisapeakinHc(d)isexplainedintheintroductionchapter,page 29 IntheinsetofFig. 22 wehaveplottedHcversus1/dfortheparticlesofsized>dcat10K.ItisclearthatHcbehaveslinearlywith1/duptoparticlesizeof24nmandthensaturates.Thisbehaviorisconsistentwiththedependenceexpectedformultidomainparticles. 38 Thusparticlesofsized>dcaremultidomainandthepeakdenesthecrossoverfromSDtoMDbehavior.Theformationofdomainstructureisdrivenbythereductionoflongrangemagnetostaticenergy,whichatequilibriumisbalancedbyshorterrangeexchangeandanisotropyenergycostsassociatedwiththespinorientationswithinadomainwall.ThepurposeofthischapteristoshowthatthiswelldenedSDregionofcoherentlyrotatingparticlesextendsoveralargerrangeofgrainsizesathighertemperaturesbecauseofthediminishinginuenceofdipolarinteractionsfromneighboringgrains. 2.4DataandDiscussion TheinuenceofdipolarinteractionsontheSD/MDcrossovercanbeunderstoodinaqualitativewaybyconsideringthethreerandomlyorientedparticlesshownschematically 36
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Figure23. Peakposition,dc,plottedasafunctionoftemperature(redcircles).Theblacksquaresaretheresultsderivedfromequation25.Thebluestarrepresentstheobservedvalueofdcforaseriesofsinglelayersamplesat10K.Theinset,aschematicofthreeneighboringparticlesorientedindierentdirections,illustrateshowthedipolareldsfromparticle2and3facilitatetheformationofdomainsinparticle1,asthedipolarmagneticeldsareindierentdirections. intheinsetofFig. 23 .Particle1experiencesdipolareldsfromparticles2and3,whicharenotcollinearformostorientationsofarandomlyorientedparticlesystem.Becausedipolareldsdecreaserapidlywithinterparticleseparation,thedipolareldduetoparticle3(2)willbestrongerthanparticle2(3)ontheleft(right)sideoftheparticle1.Theseparateandunequalinuenceoftheneighboringparticlesthusfavorstheformationofdomainsinparticle1. .Tomakethesenotionsmorequantitative,wemodifythetreatmentofDormannetal 26 forinteractingparamagnetstoincludethetemperatureregionbelowtheblockingtemperatureTBandndthetemperaturedependentdipolarmagneticeldHdarisingfromtemperatureinduceductuationsinthemagnetizationofnearestneighbornanometersizeparticlestobe, Hd=0Msa 4e(1)]TJ /F6 11.955 Tf 11.96 0 Td[(e)]TJ /F3 7.97 Tf 6.59 0 Td[(1) p (er())]TJ /F1 11.955 Tf 11.96 0 Td[(er(p )]TJ /F1 11.955 Tf 11.96 0 Td[(1))(2{1) 37
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where'er'istheimaginaryerrorfunction,Msisthesaturationmagnetization,=KV=kBT,anda=V(3cos2)]TJ /F1 11.955 Tf 13.36 0 Td[(1)=s3isadimensionlessparameterwithandscorrespondingrespectivelytoanangleparameterandtheseparationbetweentwoadjacentparticleseachwithvolumeV.TheparameterisalwaysgreaterthanoneforT
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.Intheabsenceofinteractions(Hd=0)theconditionfortheSDtoMDtransitionisgivenforsphericalparticleswithradiusd/2by,Ad3c=Bd2c,whereAd3cisthetotalmagnetostaticenergyandEdw=Bdcisthedomainwallenergy. 46 Wehaveabsorbedthefactoroftwo,whichrelatesdiametertoradius,intotheconstantsAandB.InthepresenceofthedipolarmagneticeldHd,theformationofdomainwallswillbeassistedbyaZeemantermwhichisproportionaltothevolumeoftheaectedparticle.TheconditiondeterminingtheSDtoMDtransitionnowbecomes, Ad3c=Bd2c)]TJ /F6 11.955 Tf 11.96 0 Td[(MsHdd3c=6(2{4) Whenthedipolarinteractionisasmallperturbation,i.e.,MsHd=A1,Eq. 2{1 and 2{4 canbecombinedtogivetherelation, dc=dc0)]TJ /F6 11.955 Tf 11.96 0 Td[(ddwe(1)]TJ /F6 11.955 Tf 11.95 0 Td[(e)]TJ /F3 7.97 Tf 6.58 0 Td[(1) p (er())]TJ /F1 11.955 Tf 11.95 0 Td[(er(p )]TJ /F1 11.955 Tf 11.96 0 Td[(1))(2{5) wheredc0=B=Aisthetemperatureindependentcriticaldiameterintheabsenceofinteractions(hightemperaturelimit)andddw=0BM2s=(72A2)fora==3.ThesecondtermontherighthandsideofEq. 2{5 thusbecomesatemperaturedependentcorrectiontodcduetointeractionsfromneighboringparticlesanddecreaseswithincreasingT. SincethemagneticeldduetothedipoledipoleinteractionsareweakerathighertemperaturesEq. 2{1 ,thenanoparticlesremainintheSDstatetoalargersize,whichbyEq. 2{5 resultsinashiftofdctowardshighervaluesathighertemperatures.ThisisindeedevidentinFig. 23 ,whichshowsthetemperaturedependenceofdcasdeterminedfromthedatainFig. 22 .TheblacksquaresarethesimulateddataaccordingtoEq. 2{5 usingthetwottingparameters:dc0andddw.Qualitatively,thedataagreequitewellwiththepredictionofthetheoreticalmodelwithouttakingintoaccountthetopologyandsizedistributionoftheparticles.Wehavefounddc0=84nmfromoursimulation(Fig. 23 ,blacksquares)tobeclosetothevalueforaparticlewithshapeanisotropyconstantKshape=3:1104Jm3(dc0=72AexK=0M2s,whereAexisexchangestiness, 39
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Kisanisotropyconstant). 3 ValuesofA(/0M2s)andB(/AexK)havebeenfoundtobe1.44104Jm3and1.21103Jm2respectively.ThisvalueofAisveryclosetothetheoreticalpredictedvalue 3 andthevalueofBisagainconsistentwiththevalueoftheshapeanisotropy.ThevalueoftheshapeanisotropycanalsobepredictedfromthezerotemperatureextrapolationHcoK=Msforrandomlyorientedparticles. 3 ForKshape=3:1104Jm3;Hco620Oe.Thisisingoodagreementwiththe500Oecoerciveeldobservedat10Kforthe6nmsample. Foraseparateseriesofsinglelayersamplesthecoercivitiesat10Kpeakatdc=14nmasshowninFig. 23 bythebluestar.Inthesinglelayersamplesthepeakpositionoccursathigherparticlesize(14nm)thanmultilayersamples(8nm).Thisdierencereinforcesourinterpretationandcanbeunderstoodbyrealizingthatthedipolarinteractionsofthesinglelayersamplesaresignicantlyreducedcomparedtothemultilayersamplesbecauseofthesmallernumberofnearestneighbors. 2.5Conclusion Insummary,wehavefabricatedmagneticnanoparticlesinaninsulatingthinlmmatrixwithtunablepropertiesachievedbyvaryingparticlesizeandtemperature.ThepeaksinthecoercivityisothermsdelineateacriticalgrainsizedcwhichidentiesthecrossoverfromSDtoMDbehavior.Thepresenceofdipolarinteractionsandtheirdiminishinginuencewithincreasingtemperatureisresponsiblefortheobserveddependenceofdcontemperatureandisingoodqualitativeagreementwithourmodicationofpresenttheory 26 ofinteractingparticles.Thewellestablishedinuenceofdipolarinteractionsonsuperparamagneticrelaxationtime 25 { 34 togetherwiththeconnectionbetweenrelaxationtimeandcoercivityHcsuggeststhatthereisaconcomitantinuenceofdipolarinteractionsonthecoercivityobservednearthesuperparamagneticlimitwhereHc=0.TheworkreportedhereextendsthisconnectiontotheupperlimitsonthesizeofSDparticlesbyshowingthatdipolarinteractionscanfacilitatetheformationofmultidomainparticlesespeciallyatlowtemperatures. 40
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2.6Methods 2.6.1MathematicalAnalysis TheEq. 2{5 isselfconsistent(asthetermcontainsdc)andcannotbesolvedanalytically.Theequation,dc)]TJ /F6 11.955 Tf 12.13 0 Td[(dc0+ddwe(1)]TJ /F5 7.97 Tf 6.58 0 Td[(e)]TJ /F11 5.978 Tf 5.76 0 Td[(1) p (erfi())]TJ /F5 7.97 Tf 6.58 0 Td[(erfi(p )]TJ /F3 7.97 Tf 6.59 0 Td[(1))=0,issolvedbynumericalapproachandsimultaneouslythesolutionisttedtotheexperimentaldataaccordingtoanonlinearlistsquaremethod.Mathematica,acommercialsoftware,isusedforthispurpose. 2.6.2BasicPhysicalUnderstanding AsimpliedphysicalunderstandingoftheproblemisshowninFig. 24 Figure24. Theneteectofdipolarmagneticeld(Hd)isshownontheparticle1.Asparticlesarerandomlyoriented,Hdfromparticle3willbeindierentdirectionthanthatfromparticle2.Asdipolarinteractiondecreasesrapidlywithdistance,particle1willexperiencelocaldipolarmagneticeldsindierentdirectionsfromdierentneighboringparticlesandthusmakingiteasytoformdomains. 41
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CHAPTER3EFFECTOFDIPOLARINTERACTIONONTHECOERCIVEFIELDOFMAGNETICNANOPARTICLES:EVIDENCEFORCOLLECTIVEDYNAMICS 3.1Abstract TheeectofdipolarinteractiononthecoerciveeldisdiscussedforthesingledomainandcoherentlyrotatingNinanoparticlesembeddedinAl2O3matrix.Resultsfortwosetsof5layersampleswithdierentinterlayerspacingandasetofsinglelayersamplesofNinanoparticlesarecompared.Thedipolarinteractionsarestrongestinthesampleswithshorterinterlayerdistancesandweakestforthesinglelayersamples.Inthispresentstudy,thedipolarinteractionisfoundtoincreasethecoerciveeld.Ontheotherhandthecriticalsingledomainradiusdecreasesduetothedipolarinteractions.Thesetwobehaviorstogetherindicatethatcollectivedynamicsplaysanimportantroleinunderstandingtheoriginofthecoerciveeld. 3.2Introduction Theoriginofcoerciveeld(Hc)forcoherentlyrotatingferromagneticnanoparticlesisremarkablydierentthanthatofthebulk, 47 whereirreversibledomainwallmotionisthedominantmechanism. 4 Inthecaseofnanoparticles,whenthesizeoftheparticleissmallerthanacriticalsize(dc),themostfavorableenergystateistohavesinglemagneticdomainandparticlesarecalledsingledomain(SD)particles.WhenHcisplottedasafunctionofparticlediameter(d),thereisawelldenedpeakatdc.Particleswithddc)areSD(multidomain(MD)). 2 8 41 42 44 48 Kittel 3 46 hasshownthatforasphericalparticle,dcisgivenbytherelation(seeEq. 1{3 onpage 13 ofchapter 1 ) dc=72p AK 0M2s(3{1) whereAistheexchangestiness,Kistheanisotropyconstant,0isthefreespacepermeabilityandMsisthesaturationmagnetization.InSDparticlesthereisnodomainwall.TheoriginofHcinthiscaseisthenitetimerequiredtoreversethemagnetizationdirectionoverthemagneticelddependentanisotropyenergy. 47 Thetimerequiredto 42
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reversethedirectionofthemagnetizationofacoherentlyrotatingSDparticleisgivenbytherelation 2 5 49 50 =0expKV kBT:(3{2) Here,0istheinverseoftheattemptfrequencytoovercometheenergybarrier,Visthevolumeoftheparticle,kBistheBoltzmannconstantandTisthetemperature.StonerandWohlfarthhavecalculatedHcforSDparticlesinthesimplecasewhenparticlesarecoherentlyrotatingandtheappliedmagneticeldisalongtheeasyaxisofmagnetizationoftheparticles.ThecoerciveeldforaStonerWohlfarthparticleisgivenby HcSW=2K Ms241)]TJ /F8 11.955 Tf 11.95 20.44 Td[( ln(m 0) ln( 0)!1 235;(3{3) wheremisthetimeofmeasurement.FromthesimpleStonerWohlfarthmodelitisclearthatHcforthenanoparticlecandependonmanydierentfactors.Hcincreaseswithdecreasingm,increasingandincreasingK. Inthepresenceofdipolarinteractionstheaboveequationwillbemodied.Thewidelyacceptedmodicationisachievedbytreatingthedipolarinteractionstoresultinaneectiveanisotropyenergy. 51 { 61 .ThusifduetothedipolarinteractionsKincreases(decreases)then,accordingtoEq. 3{2 ,willalsoincrease(decrease)andasanetresultHcwillincrease(decrease).AmorefamiliarfamousformofEq. 3{3 isHcSW(T)=2K=Ms(1)]TJ /F1 11.955 Tf 12.13 0 Td[((T=TB)1=2),whereTB=KV=25kBistheblockingtemperature.Thefactor25comesfromthefactthatm100sisatypicalmeasurementtimeand)]TJ /F3 7.97 Tf 6.58 0 Td[(10109sec)]TJ /F3 7.97 Tf 6.58 0 Td[(1isatypicalattemptrate. Theeectofdipolarinteractiononthecoerciveeld(Hc)hasbeeninvestigatedextensively.ThersttheoreticaltreatmentbyNeel 62 showedthatHcdecreaseswiththeincreaseinthepackingfraction()orthedipolarinteractionasshownbelowinEq. 3{4 ,wheretheinteractioneecthasbeenintroducedasan"InteractionField"andshownto 43
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lowertheanisotropyenergy. Hc=Hc1(1)]TJ /F6 11.955 Tf 11.95 0 Td[()(3{4) The"InteractionField"isafunctionofthepackingfraction().LaterWohlfarth 51 showedthattheeectoftheinteractionontheHccanbeincreasingordecreasingdependingontheparticleorientationasthedipolarinteractionisdirectiondependent.Butallofthoseresultshavebeenconstructedconsideringthefactthattheanisotropyconstant,K,eitherincreasesordecreasesduetotheinteractions.PrevioustheoreticalandexperimentalworkshavebeenreportedeithershowinganincreaseordecreaseinHcandexplainedintermsofacorrespondingincreaseordecreaseintheanisotropyenergy. 51 { 61 63 InthispresentexperimentwendthatanincreaseinthedipolarinteractionincreasesHcbutdecreasesdc.Equation 3{1 suggeststhatthedecreaseindcmaybeduetoadecreaseintheK.ButadecreaseintheKwillalsodecrease(Eq. 3{2 )andthuswilldecreaseHc(Eq. 3{3 )whichiscontradictorytothepresentexperimentalresult.ThusthechangeofKduetothedipolarinteractionsmustnotbeapplicableinthepresentcase.AsanychangeinKwillgiverisetochangeinHcanddcbothinthesamedirection(bothincreaseordecreaseatthesametime).Below,weshowqualitativelythattheincreaseintheHccanberealizedintermsofthecollectivedynamicsofthemagnetizationoftheparticlesanddecreaseindccanbeunderstoodasdiscussedinreference 48 3.3ResultsandDiscussions Samplesweregrownusingpulsedlaserdepositiontechnique. 48 Basepressureofthegrowthchamberwasontheorderof10)]TJ /F3 7.97 Tf 6.58 0 Td[(7Torrandthegrowthtemperaturewasaround550oC.MultilayerstructureofAl2O3andNinanoparticleweregrownwithoutbreakingthevacuumofthechamber.Firstathick(40nm)buerlayerofAl2O3isgrownontopofthesubstrate.ThepurposeofthisbuerlayeristopreventanydiusionoftheNiintothesubstrate.ThenNinanoparticlesandAl2O3aresequentiallydepositedonthisbuerlayer(seeFig.1).ThetoplayerofAl2O3actsasacappinglayerwhichpreventsoxidationofthenanoparticles. 36 Threedierentsetsofsamplesaregrown.Set1andset2samples 44
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consistof5layersofNinanoparticlesseparatedbyAl2O3layers.Forset1(set2)theAl2O3separationis3nm(40nm).Set3samplesaresinglelayerofNinanoparticlesinAl2O3matrix.Dipolarinteractionsarestrongestinset1,moderateinset2andweakestinset3.ThedipolarinteractionsarestrongerinSet1comparedtoset2astheinterlayerseparationoftheNiparticlesissmallerinset1comparedtoset2.Set3consistsofonlyasinglelayerofNiparticlesandthusthedipolarinteractionsareweakest.Allsetsofsamplesconsistofdierentsampleswithvaryingparticlesizefrom3nmto60nm. Figure31. Fig1a)showstheTEMimageofasinglelayersamplewithaverageparticlediameterof24nm.Particlesarewelldenedwithinterparticledistanceofaround4nm.1b)showsaschematicofthesinglelayersample.A40nmthickbuerlayerofAl2O3isrstgrownontopofsubstrate.ThentheNinanoparticlesaregrownontoofthebuerlayer.Finallya3nmthickcappinglayerofAl2O3isgrowntoprotectitfromoxidation.1c)showstheschematicof5layersofNinanoparticlesample. Figure 31 a)showstheTEMimageofthesinglelayerNiparticleswithaverageparticlediameterof24nm(set3).Thesimpliedschematicofthesingleandmultilayersamplesareshownin 31 b)andc). TypicalmagnetizationloopsatthreedierenttemperaturesareshowninFig. 32 a)forthesamplewith3nmAl2O3spacerlayer(set1)and6nmindiameter.ThecoerciveeldHc(T)isdeterminedfromtheloopasshownbythearrow.ThisproceduretodetermineHcisrepeatedforallsamplesbelongingtoallthreesets.Attemperatures 45
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Figure32. a)Magnetizationloopofasamplefromset1ofaverageparticlediameterof6nm.Coerciveeld(Hc)isdeterminedfromtheloopasshownbythearrow.Hcdecreaseswithincreasingtemperatureandgoestozeroabovetheblockingtemperature.b)Magnetizationloopsaboveblockingtemperatures.MagnetizationisplottedasthefunctionofH=TtoshowthesuperparamagneticbehaviorasexpectedfortheSDparticlesabovetheblockingtemperature. abovetheblockingtemperatures(TB)SDsamplesbehaveassuperparamagneticparticles.Figure 32 b)showsthesuperparamagneticbehavioroftheset1,6nmdiametersample.NotethemagnetizationdatafallontopofeachotherwhenplottedasafunctionofH=T.ThisbehaviorisadirectconsequenceofthesuperparamagneticbehaviorasexpectedfromthecoherentlyrotatingSDparticles. Figure 33 showsHcplottedasafunctionofdfortheset1,set2andset3samples.Thedatathatcorrespondtothedierentsamplesetsareindicatedinthelegends.ThepeakintheHcseparatesSDandMDparticles. 2 8 41 42 44 48 Itisclearfromthedatathatdcdecreaseswithincreasingdipolarinteractions(dc1
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Figure33. Coerciveeld(Hc)asafunctionofparticlediameter(d).Thepeakseparatesthesingledomain(SD)andmultidomain(MD)particles.Particleswithdiameterhigher(smaller)thanthepeakdiameter(dc)areMD(SD).Dataforthe3dierentsamplesetsareshownandindicatedinthelegends.Thecriticaldiametersdc1,dc2,dc3areshownfromthesamplesofset1,set2andset3respectively.Inthesingledomainregion(belowdc)thecoercivityincreaseswithincreasingdipolarinteractionsasshownbytheverticaldottedarrow. magnetizationduetothedipolarinteractionsisfoundtoberesponsiblefortheincreaseinHc.TheseobservationsareshowninFig. 33 andsummarizedinFig. 34 WerstdiscusstheeectofdipolarinteractionsonHcaspresentedinpreviousinvestigations. 51 { 61 ThetreatmentbeginbyincludingthechangeinanisotropyenergyEdip,duetodipolarinteractionintotheexpressionfor,asgivenby 63 =0expKVEdip kBT(3{5) 47
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Equation 3{5 canberewrittenasshowninEq. 3{6 .Thustheeectofthedipolarinteractionsistreatedaseitheranincrease(+Edip)ordecrease(Edip)ofanisotropyenergy. =0expK(eff)V kBT(3{6) TheeectofdipolarinteractionsontheHccanbeexplainedaccordingtoEq. 3{6 .Inourcasea+Edipincreases+andgiverisetoanincreaseinHcwithincreasingdipolarinteractions(Eq. 3{2 and 3{3 ).IfthisistobetrueinourcasethenaccordingtoEq. 3{1 ,dcshouldalsoincreasewithincreasingdipolarinteractions.AccordingtothepreviousapproachbothHcanddcshouldchangeinthesameway,bothincreaseorbothdecrease.InthepresentexperimentwendhoweverthatHcincreasesanddcdecreasesduetodipolarinteractions(seeFig. 34 )andstronglysuggestsanalternativeapproachtotheproblem.Theeectofdipolarinteractionsondcisdiscussedinreference 48 ,whereithasbeenshownthatthelocaldipolarmagneticeldfromthenearbyrandomlyorientedparticlestrytoalignthemagnetizationdirectionoftheparticleindierentdirectionsandthusfavoringdomainformation.TheeectofdipolarinteractionsonHcwillbediscussedbelowintermsofcollectivedynamics. Itiswellknownthatthemagnetizationdynamicscanbecollectiveinnatureduetotheinteractionsbetweentheparticlesandtherelaxationtime()inthiscaseisgivenby 64 65 =T Tg)]TJ /F1 11.955 Tf 11.95 0 Td[(1)]TJ /F5 7.97 Tf 6.58 0 Td[(z;T>Tg(3{7) whereistherelaxationtimeofthesinglenoninteractingparticle(Eq. 3{2 ),Tg=0M2=4kBr3isthecriticaltemperatureanddependsontheinterparticledistanceandparticlemagnetizationandzisacriticalexponent.TheaboveequationclearlysuggeststhattherelaxationtimewillbelargerinthepresenceofdipolarinteractionsandthusaccordingtoEq. 3{3 Hcwillbelarger,andthusagreeingwithourexperimental 48
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Figure34. Coerciveeld(Hc)andcriticaldiameter(dc)asthefunctionoftheincreasingdipolarinteraction.Hc(dc)increases(decreases)withincreasingdipolarinteraction.TheoppositebehaviorofHcanddcsuggeststhatthecollectivedynamicsandthecriticalslowdownisresponsiblefortheincreaseinHcduetothedipolarinteractions.Thedecreaseindcisdiscussedelsewhere. 48 observations(Fig. 34 ).Notethatinthiscasetheanisotropyenergyisunaectedbydipolarinteractionsandtheincreaseinrelaxationtimeisduetothefactthatthereversalofmagnetizationiscollectiveinnature. 64 65 3.4Conclusions AstudyofdipolarinteractionsispresentedforthesingleandmultilayerstructureofNinanoparticles.Thecoerciveeldhasbeenfoundtoincreasewithincreasingdipolarinteractionsandcanbeunderstoodqualitativelyintermsofcollectivedynamics.Threesetsofsamplesareinvestigated.Eachsetconsistsofsampleshavingparticlesizevaryingfrom3nmto60nmindiameter.Dipolarinteractionsarestrongerinset1anddecreasesforset2andset3.Behaviorofcoerciveeldandcriticalsingledomainradiusareobserved.Coerciveeldincreasesandcriticalsingledomainradiusdecreases 49
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withincreasingdipolarinteractions.ThesetwobehaviorstogethersuggestacollectivedynamicsofthemagnetizationreversalprocessintheSDregioninthepresenceofdipolarinteractions.Toourknowledge,thisisthersttimethattheeectofcollectivedynamicsonacoerciveeldofthenanoparticlesystemhasbeenobserved. 50
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CHAPTER4FINITESIZEEFFECTSWITHVARIABLERANGEEXCHANGECOUPLINGINTHINFILMPD/FE/PDTRILAYERS 4.1Abstract ThemagneticpropertiesofthinlmPd=Fe=Pdtrilayersinwhichanembedded1.5AthickultrathinlayerofFeinducesferromagnetisminthesurroundingPdhavebeeninvestigated.ThethicknessoftheferromagnetictrilayeriscontrolledbyvaryingthethicknessofthetopPdlayeroverarangefrom8Ato56A.AsthethicknessofthetopPdlayerdecreases,orequivalentlyastheembeddedFelayermovesclosertothetopsurface,thesaturatedmagnetizationnormalizedtoareaandtheCurietemperaturedecreasewhereasthecoercivityincreases.ThesethicknessdependentobservationsforproximitypolarizedthinlmPdarequalitativelyconsistentwithnitesizeeectsthatarewellknownforregularthinlmferromagnets.Thefunctionalformsforthethicknessdependences,whicharestronglymodiedbythenonuniformexchangeinteractioninthepolarizedPd,provideimportantnewinsightstounderstandingnanomagnetismintwodimensions. 4.2Introduction Thepresenceof3dmagnetictransitionmetalionsinpalladium(Pd)givesrisetogiantmomentsthussignicantlyenhancingthenetmagnetization 66 { 70 .PdisknowntobeinthevergeofferromagnetismbecauseofitsstrongexchangeenhancementwithaStonerenhancementfactorof10 71 .ThemagneticimpuritiesinducesmallmomentsonnearbyPdhostatomstherebycreatingacloudofpolarizationwithanassociatedgiantmoment 71 72 .Neutronscatteringexperimentsshowthatthecloudofinducedmomentscaninclude200hostatomswithaspatialextentintherange10to50A 72 73 .ThusathinlayerofFeencapsulatedwithinPdwillbesandwichedbetweentwoadjacentthinlayersofferromagneticPdwithnonuniformmagnetizationandatotalthicknessintherange20to100A. 51
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WehaveinvestigatedthinlmPd/Fe/PdtrilayersinwhichthethicknessdFeoftheFeisheldconstantnear1.5AandthethicknessofthepolarizedferromagneticPdisvariedbychangingthetopPdlayerthicknessx.Themagneticpropertiesarestudiedasafunctionofx.Ourexperimentsaremotivatedbytherecognitionthatferromagnetisminrestricteddimensionshasattractedsignicantresearchinterest 74 { 78 .Forexample,thecoerciveeldHcincreasesasthethicknessoftheferromagneticlmisdecreasedtowardathicknesscomparabletothewidthofatypicaldomainwall 79 80 .Moreover,theCurietemperatureTcdecreasesasthethicknessoftheferromagneticlmisdecreasedtowardathicknesscomparabletothespinspincorrelationlength 81 { 83 .WewillshowbelowthatsimilarphenomenologyappliestoferromagneticallypolarizedPdlms,albeitwithdierentfunctionaldependencesarisingfromthefactthatexchangecoupling,whichdecayswithdistancefromtheferromagneticimpurity 84 ,isnotuniformthroughoutthelm. 4.3ExperimentalDetails ThesamplesweregrownonglasssubstratebyRFmagnetronsputtering.Thebasepressureofthegrowthchamberwasoftheorderof10)]TJ /F3 7.97 Tf 6.58 0 Td[(9Torr.FirstathicklayerofPdofthickness200Aisgrownontopofthesubstrate.TherootmeansquaresurfaceroughnessofthisPdlayerwasmeasuredbyatomicforcemicroscopytobe6A.Thenaverythin(1.5Aasrecordedbyaquartzcrystalmonitor)layerofFeisdepositedontopoftherstPdlayer.FinallyatoplayerofPdwiththicknessxisgrowntocompletethetrilayerstructureshownschematicallyinFig. 41 a.WediscusssixdierentsampleswiththetopPdlayerhavingathicknessxvaryingfrom8to56A.ThetotalthicknessyofthepolarizedPd(seeFig. 41 b)canrangefrom20to100A 72 73 .Thusforx
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Figure41. a)MultilayerstructureofaPd/Fe/Pdtrilayer.ThebottomlayerofPdis200Athick.ThethicknessoftheFelayeris1.5Aasrecordedbythequartzcrystalmonitor.ThethicknessxofthetoplayerofPdisvariedfrom8to56A.b)Magneticstructureofthesample.ThetotalthicknessyofpolarizedPdisintherange20to100A(shadedredarea).Thusbyvaryingx,itispossibletovarythethicknessyofthepolarizedferromagneticPdlayer.c)IntensityofFe3(703.0eV)LMMAugerelectronpeakplottedasafunctionofmaterialremovedbyargonsputtering.Thedata(solidblackcircles)arettoaGaussiandistribution(redline).Thefullwidthhalfmaximumvalueof1.85Aisconsistentwithcrystalmonitormeasurements AugerelectronpeakofFig. 41 cshowsthattheFeisembeddedinthePdasadistinct2DlayerwithaFWHMthicknessof1.8A.Allofthesestepswereperformedwithoutbreakingvacuum.MeasurementsofthemagnetizationM(Fig. 42 )wereperformedusingaQuantumDesignMPMSsystem.ThemagneticeldHwasalongtheplaneofthesubstrate.Sincethemagnetizationmeasurementswereexsitu,xwasconstrainedtobegreaterthan8A;otherwisetheexposureofthesampletoaircausedunwantedoxidationoftheFe.ThemagneticparametersHc(x)(Fig. 43 )andTc(x)(Fig. 44 )arecalculatedrespectivelyfrommagnetizationloopstakenat10K(seeinsetofFig. 43 )andlinearextrapolationsofthetemperaturedependentmagnetizationtakenatH=20Oe(seeinsetofFig. 44 ).ThemagneticcontributionfromthebottomferromagneticPdlayerisindependentofx,sincey=2<200A,theconstantthicknessofthebottomlayer. 53
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Figure42. ThesaturationmagnetizationnormalizedtotheareaofthesampleMsAshowsasmoothincreasewithincreasingthicknessx.Theexperimentaldataareshownassolidblackcirclesandthedashedblacklineisaguidetotheeye.Saturationtoaconstantvalueoccursnear30A(verticalarrow). 4.4ResultsandDiscussion Forlargevaluesofx,thethicknessyofthecombinedpolarizedferromagneticPdlayersandtheassociatedsaturatedmagnetizationM=Mswillreachaconstantvalue.ThisexpectationisborneoutinFig. 42 whichshowsthexdependenceofsaturatedmagnetizationMsAnormalizedtosamplearea.WenotethatthisnormalizedsaturatedmagnetizationMsA(x)increaseswithincreasingxasthetotalamountofpolarizedPdincreases.Theonsetofsaturation,nearx=30AindicatesthatthepolarizationcloudincludingtheembeddedFelayeris60Athick.Thisvalueisconsistentwithpreviousobservation 73 .TheincreaseofMsAwithxshowninFig. 42 isthusstraightforwardtounderstand.AsxincreasesthethicknessofthetoppolarizedferromagneticPdlayerincreaseswithaconcomitantincreaseofmagneticmaterialinthesystem.VariationofxclearlycontrolsthethicknessofthepolarizedferromagneticPdlayer.Whennormalizedto 54
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Figure43. ThecoerciveeldHcshowsastrongincreaseasthethicknessxofthetoplayerofthePddecreases.Thedataareshownassolidblackcirclesandtheblacksolidlineisapowerlawtwithexponent=2:3(0:1).TheinsetshowsmagnetizationloopsatT=10Kforx=8A(solidblacksquares)andx=56A(solidredcircles). thenumberofFeatomspresent,thesaturatedmagnetizationMsA=1:110)]TJ /F3 7.97 Tf 6.59 0 Td[(4emu/cm2correspondsto9.2BperFeatom,incloseagreementwithpreviousobservationsofthegiantmomentofFeinPdtobenear10B 72 .ModelingthexdependenceofMsA(x)showninFig. 42 forourPd=Fe=Pdtrilayersisnotstraightforward.ForregularferromagnetswithMsuniformthroughoutthethickness,wewouldexpectMsA(x)tobelinearinx;clearlyitisnot.AreasonablemodelwillincorporateanexchangeinteractionJthatdecaysradiallywiththedistancefromthepointferromagneticimpurity 84 .ThiscomplicationrequiresmodelingJasafunctionofdistancexfromtheplaneofimpurity.AstartingpointwouldbetowritethemagnetizationMisafunctionofJ 4 M(H;T;x)=MsBs Ms kBT"gBH+2pMJ(x)#!;(4{1) 55
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Figure44. TheCurietemperatureTcrapidlyincreaseswithincreasingx.Dataareshownassolidblackcirclesandthedashedblacklineisaguidetotheeye.Saturationtoaconstantvalueoccursnear20A(verticalarrow)TheinsetwithTcindicatedbytheverticalarrowshowsthetemperaturedependentmagnetizationtakeninaeldH=20Oe. whereBsistheBrillouinfunctionandpisthenumberofthenearestneighborsbeyondwhichJiszero.InprincipletheexperimentallydeterminedvaluesofM(H;T;x)canbettoEq. 4{1 tondthebesttvaluesofJ(x)fordierentvaluesoftheparameterp.Wehavenotperformedsuchananalysis. Fig. 43 showsthebehaviorofthecoercivityHc(x)asafunctionofx(solidblackcircles).Thedataarewelldescribedbyapowerlawdependence(solidblackline),Hc(x)/x)]TJ /F5 7.97 Tf 6.58 0 Td[(,wheretheexponent=2:3(0:1)isclosetotheratio7/3.Similarpowerlawbehaviorrevealsitselfinregularferromagneticthinlmswherehasasomewhatsmallervaluevaryingfrom0.3to1.5 76 .Becausedependsstronglyonstrain,roughness,impurity,andthenatureofthedomainwall(BlochorNeeltype) 76 ,itisnotsurprisingtoseeawidevariationin.NeelpredictedforexamplethatforBlochdomainwalls,Hcofaferromagneticthinlmshouldvaryasx)]TJ /F3 7.97 Tf 6.59 0 Td[(4=3whenthethicknessxofthelm 56
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iscomparabletothedomainwallthicknessw 79 .ForthecaseofNeelwalls,Hcdependsonlyontheroughnessofthelmanddoesnotdependonlmthickness 77 .ThevariationofHc(x)becomesparticularlypronouncedwhenthelmthicknessbecomescomparabletow. AqualitativeunderstandingofthesteeperHc(x)dependencebecomesevidentbyrecognizingthattheformationofdomainstructureisdrivenbythereductionoflongrangemagnetostaticenergywhichatequilibriumisbalancedbyshorterrangeexchangeandanisotropyenergycostsassociatedwiththespinorientationswithinaBlochorNeeldomainwall.Domainwallthicknessisgivenbyw=p A=K 3 82 whereKisthecrystallineanisotropyconstantandAistheexchangestiness,proportionaltotheexchangeenergy,J 85 .ThedomainwallsizewincreasesfordecreasingKandincreasingJ.IfK,whichdependsontherelativelyconstantspinorbitinteraction 4 withinthePdcomponentofthePd=Fe=Pdtrilayers,remainsconstant,thenvariationsinwaredominatedbyvariationsinJ.Thusasxdecreasestowardzero,theincreaseinJ 84 givesrisetoanincreaseinwwhichinturngivesrisetoamorerapidincreaseinHcthanwouldbeseeninregularferromagnetswithconstantJ.Asdiscussedabove,thisrapidvariationwith7=3isobservedexperimentally. ThedatainFig. 44 showthatTcincreasesasxincreasesandreachesarelativelyconstantvaluenearx=20A.ThedashedblacklineisaguidetotheeyeandisqualitativelysimilartothebehaviorofMsA(x)showninFig. 42 whichsaturatesatalargervaluenear30A.Theseobservationsareagainqualitativelyconsistentwiththenitesizeeectassociatedwithcriticalphenomenainferromagnets 81 { 83 .Althoughthedataarenotofsucientqualitytodistinguishthepowerlawbehaviorthatispredictedfornitesizeeects 81 { 83 ,weexpectthatthedependenceisfurthercomplicatedbythepreviouslydiscusseddependenceofJonxinpolarizedferromagneticPd.ThebehaviorofTc(x)suggeststhatPd=Fe=Pdtrilayershouldbetreatedasasinglelayerwithawelldenedspinspincorrelationlength.IfthePdlayersaretreatedseparately,thenthebottomlayer 57
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withxedthicknessy=2wouldhaveaTcequaltothehighestTcofthetoplayer.InthiscasetheoverallmeasurementwouldnotshowastrongchangeinTcasafunctionofx,sincetheTcofthebottomlayerwoulddominateforallx. Wenotethatforourplanargeometry,TcdecreaseswithdecreasingthicknessashasalsobeenshownforthinlmNi 81 andepitaxialthinlmstructuresbasedonNi,CoandFe 82 .OntheotherhandTcincreaseswithdecreasingsizeofferrimagneticMnFe2O4nanoscaleparticleswithdiametersintherange526nm 83 .ThisincreaseofTcwithdecreasingsizeisattributedtonitesizescalinginthreedimensionswhereallthreedimensionssimultaneouslycollapse 83 .Inourtwodimensionalplanarthinlmsonlyoneofthedimensions,thethickness,collapsesandTcdecreasesratherthanincreasesinaccordwiththeobservationsofpreviousstudies 81 82 4.5Conclusions Inconclusion,wehavecharacterizedthemagneticpropertiesofthinlmPd=Fe=Pdtrilayersanddeterminedthatcriticalsizeeectsapplyto\ferromagnetic"PdwheretheferromagnetismisinducedbyproximitytoanunderlyingultrathinFelm.Thecriticalsize,orequivalentlythecriticalthickness,iscontrolledbyvaryingthethicknessxofthetopPdlayer.ThedependencesonlmthicknessofthecoerciveeldHcandtheCurietemperatureTcareinqualitativeagreementwithnitesizeeectsseeninregularferromagneticlmswheretheexchangecouplingJisconstantthroughoutthelm.TheresultspresentedhereincreaseourunderstandingofnanomagnetisminultrathinsystemsbyshowingthatthespatialvariationsofJintheproximitycoupledPdhaveapronouncedinuenceontheformofthicknessinducedvariations,namely:anonlineardependenceofMsA(x),anunusuallystrongpowerlawdependenceofHc(x)andadependenceofTc(x)whichindicatesthatthetrilayeractsasasinglelayerthatnecessarilyincludestheconstantthicknessPdlayerservingasasubstratefortheFelayer. 58
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CHAPTER5TEMPERATUREDEPENDENCEOFCOERCIVITYINMULTIDOMAINNINANOPARTICLES,EVIDENCEOFSTRONGDOMAINWALLPINNING 5.1Abstract Thetemperaturedependenceofthecoercivityofthesingleand5layersamplesofNinanoparticlesinAl2O3matrixisstudied.AlinearT2=3dependenceofcoercivityoverawiderangeoftemperature(10Kto350K)isobserved.Allthesamplesconsistsofparticleswithmultiplemagneticdomainsasthesizeoftheparticlesarelargerthanthecriticalsingledomainsize(seeEq. 1{3 onpage 13 ofchapter 1 andFig. 33 onpage 47 ofchapter 3 ).Theexperimentalresultsareunderstoodintermsofstrongdomainwallpinning. 5.2Introduction Thetemperaturedependenceoftheextrinsicmagneticproperties,forexamplecoerciveeld(Hc(T)),arisefromtwomechanisms.Therstmechanismis,duetothetemperaturedependenceoftheintrinsicmagneticproperties 11 15 86 87 suchassaturationmagnetization(Ms),magneticanisotropy(K)andexchangestiness(A)andwillbediscussedinchapter 6 .Thesecondmechanismis,duetothethermallyactivatedhopingofthemetastablestatesoversomeenergybarrier. 2 { 4 6 Fromthemagnetizationloopsatdierenttemperatures(Fig. 52 )wehavefoundthatMsdoesnotchangewithtemperature.Allthesamplescomprisepolycrystallineparticles 36 andthusmagnetocrystallineanisotropycanbeneglectedandtemperatureindependentshapeanisotropyisdominant. 48 Theexperimentaltemperaturerangeis10Kto300KwhichismuchsmallerthanthecurietemperatureofNi(630K) 3 andAcanbeconsideredconstantoverthistemperaturerange. 88 Inthischapterwewilldiscussthesecondmechanismastheoriginofthetemperaturedependenceofthecoerciveeld(Ms,KandAaretemperatureindependent).TounderstandthetemperaturedependenceoftheHcduetothethermallyactivatedhoppingovermetastableenergyminimaseparatedbysomeenergybarrier,itisnecessarytondoutthemagneticelddependenceoftheenergybarrier.Acommonly 59
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usedphenomenologicalenergybarrieris 2 3 47 89 E=E0[1)]TJ /F6 11.955 Tf 11.96 0 Td[(H=Hc0]m(5{1) whereE0istheenergybarrieratzeromagneticeldandenergybarriervanishesatH=Hc0atT=0.AtH=Hc,thermalenergy,kBT,issucientlyhightocausemostofthemomentstobethermallyactivatedoverthebarrier.ForexampleforthecaseofStonerWohlfarthparticlesm=2,E0=KVandHc0=2K=Ms.ForStonerWohlfarthparticlesthescenarioisverysimpleandtheEq. 5{1 canbederivedanalytically(seeEq. 1{6 onpage 15 ofchapter 1 ).RememberthatifE(H)isknown,itispossibletocalculateHc(T).InthischapterwewilldiscusshowtoderiveE(H)(Eq. 5{1 )fortheMDnanoparticlesandwillcompareHc(T)withthemodel. 5.3ResultsandDiscussions Thesamplepreparationtechniqueisdiscussedinchapter2andchapter3.Threedierentsetsofsamplesareinvestigated.Set1consistsofsinglelayerNiparticlesinanAl2O3matrix.Set2andSet3consistsof5layersofNiparticlesseparatedbyAl2O3layers.TheinterlayerseparationinSet2andSet3are3nmand40nmrespectively.TheschematicofallthreesetsofsamplesareshowninFig. 51 below. InthischapterwewillfocusonthetemperaturedependenceofHcfortheMDNinanoparticles.Atotalof15samplesarestudied,5samplesfromeachset.Magnetizationloopsaremeasuredforeverysampleforseven(onaverage)dierenttemperatures.Thismeansatotalofaround105magnetizationloopshavebeenmeasuredforthepresentstudy.Magnetizationloopsforthesampleofaverageparticlediameterof12nmofset2atdierenttemperatures(indicatedinthelegends)areshowninFig. 52 .ThearrowshowsHcat10K.NotethatHcdecreaseswithincreasingtemperature.ThetemperaturedependenceofHcnormalizedtoHcOforvedierentsamplesbelongingtoset1isshowninFig. 53 .Theparticlediametersareindicatedinthelegends.NoteT2=3inxaxis.AllthedatafollowalinearT2=3dependence.Tounderstandtheabovedata,wewillstart 60
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Figure51. Schematicofthreesetsofsamples.Set1comprisesasinglelayerofNiparticlesembeddedinanAl2O3matrix.Set2andSet3comprisesof5layersofNiparticlesseparatedbydierentdistancesinanAl2O3matrix.TheinterlayerdistancesinSet2andSet3are3nmand40nmrespectively. withageneralmagneticenergylandscapeofthesystemwrittenasapolynomialexpansionofthedomainwallposition(x)aroundastrongpinningcenter. 2 { 4 6 E(x)=a0+a1x+a2 2x2+a3 3x3)]TJ /F6 11.955 Tf 11.95 0 Td[(b0Hx(5{2) wherea0,a1,a2,a3andb0aremicromagneticparametersthatdependonthemagneticparametersK,MsandA.Forthestrongpinningcenterthex3termisincludedastheeectofthepinningcenterislongdistancecomparedtotheweakpinningcenterwherethex3termisneglected. 3 Therelationbetweenmicromagneticandmagneticparametercanbedeterminedfromtheparticularmodelused.Notethatthemicromagneticparametersaretemperatureindependentinourcaseastheyonlydependonthetemperatureindependentmagneticparameters.First,wewillderivetheenergybarrierseparatingthemetastableminimafromtheglobalminima.ThemaximaorminimaofE(x)aredeterminedbysettingtherstorderderivativetozero. E x=a1+a2x+a3x2)]TJ /F6 11.955 Tf 11.95 0 Td[(b0H=0(5{3) 61
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Figure52. Magnetizationloopsforthesampleofaverageparticlediameterof12nmofset2atdierenttemperatures(indicatedinthelegends).Thecoerciveeld(Hc)at10Kisindicatedbythearrow.Hcdecreaseswithincreasingtemperature.Saturationmagnetization(Ms)isconstantatdierenttemperatures. Thetwosolutionsfortheaboveequationsare x1=)]TJ /F6 11.955 Tf 9.3 0 Td[(a2+p a22)]TJ /F1 11.955 Tf 11.96 0 Td[(4a3(a1)]TJ /F6 11.955 Tf 11.96 0 Td[(boH) 2a3(5{4) x2=)]TJ /F6 11.955 Tf 9.3 0 Td[(a2)]TJ /F8 11.955 Tf 11.96 10.37 Td[(p a22)]TJ /F1 11.955 Tf 11.95 0 Td[(4a3(a1)]TJ /F6 11.955 Tf 11.96 0 Td[(boH) 2a3(5{5) TakingthesecondderivativeofE(x)withrespecttoxitiseasytoshowthat2E=x2jx1>0(2E=x2jx2<0)andcorrespondstothemaximum(minimum).Thustheenergybarrieris E(H)=E(x1))]TJ /F6 11.955 Tf 11.95 0 Td[(E(x2)=(a22)]TJ /F1 11.955 Tf 11.95 0 Td[(4a1a3+4a3b0H)3=2 6a23(5{6) 62
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Figure53. Coerciveeld(Hc)vs.T2=3forvedierentsamplesofset1.Thelinearbehaviorisobservedforsampleswithparticlesizefrom18nmto42nmindiameter. Forthereverseeld,ieH=)]TJ /F6 11.955 Tf 9.3 0 Td[(Htheaboveequationreducesto E(H)=(a22)]TJ /F1 11.955 Tf 11.95 0 Td[(4a3(a1+b0H))3=2 6a23=(a22)]TJ /F1 11.955 Tf 11.95 0 Td[(4a1a3)3=2 6a23 1)]TJ /F6 11.955 Tf 27.42 8.09 Td[(H a22)]TJ /F3 7.97 Tf 6.59 0 Td[(4a1a3 4a3b0!3=2 (5{7) whichisinthesameformofEq. 5{1 ,where E0=(a22)]TJ /F1 11.955 Tf 11.95 0 Td[(4a1a3)3=2 6a23(5{8) Hc0=a22)]TJ /F1 11.955 Tf 11.95 0 Td[(4a1a3 4a3b0(5{9) FromEq. 5{7 itisclearthatE(H)decreaseswithincreasingHandwhenH=Hctheenergybarriercanbeovercomebythermalenergy(denitionofthecoerciveeld).Thus 63
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atH=Hc,theEq. 5{7 canberewrittenas kBT=(a22)]TJ /F1 11.955 Tf 11.95 0 Td[(4a1a3)3=2 6a23 1)]TJ /F6 11.955 Tf 25.8 8.09 Td[(Hc a22)]TJ /F3 7.97 Tf 6.59 0 Td[(4a1a3 4a3b0!3=2(5{10) TheaboveequationcanbesolvedforHc Hc=Hc0"1)]TJ /F8 11.955 Tf 11.95 16.86 Td[(kBT E02=3#(5{11) whereHc0andE0aregivenbyEq. 5{8 and 5{9 .ThistemperaturedependenceofHcisconsistentwiththeexperimentalresultsshowninFig. 53 54 and 55 Figure54. Coerciveeld(Hc)vs.T2=3forvedierentsamplesofset2.Thelinearbehaviorisobservedforsampleswithparticlesizefrom12nmto60nmindiameter. 64
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Figure55. Coerciveeld(Hc)vs.T2=3forvedierentsamplesofset3.Thelinearbehaviorisobservedforsampleswithparticlesizefrom16nmto44nmindiameter. 5.4RelationBetweenMicromagneticParameterandMagneticParameters Herewewilloutlinearoadmaptorelatethemicromagneticparametersa0,a1,a2,a3andb0tothemagneticparametersK,MsandA.Todothatwewillstartwiththemagneticenergyexpression, 3 E(x)=Z"ArM(x) Ms2)]TJ /F6 11.955 Tf 11.96 0 Td[(K(x)(k:M(x))2 M2s)]TJ /F6 11.955 Tf 11.96 0 Td[(0M(x):H)]TJ /F6 11.955 Tf 13.15 8.09 Td[(0 2M(x):Hd(M)#dV(5{12) wherethersttermcorrespondstotheexchangeenergycostduetothespinmisalignment,thesecondtermistheanisotropyenergy,thethirdtermistheZeemanenergyandthefourthtermisthemagnetostaticselfenergy.Thepositionofthedomainwallisgivenbyxandkistheunitvectoralongtheeasyaxis.Theaboveequationshouldbesolvedforreal 65
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sampleswhiletakingintoaccountrealstructureandimperfections.Therealstructureandimperfectionsareresponsibleforthexdependenceofthemagneticparameters(Ms(x),A(x),K(x)).AftersolvingEq. 5{12 andbycomparingthecoecientsofthedierentpowerofx,itispossibletondoutthemicromagneticparametersintermsofmagneticparameters.ThebehaviorsofHc0andE0=kBareshowninthegurebelow. Figure56. ThebehaviorsofHc0andE0onparticlediameterareshownforset2samples.Hc0decreasesandE0=kBincreaseswithincreasingparticlesize. TheincreasingbehaviorofE0anddecreasingbehaviorofHc0areconsistentwiththeliterature. 3 Theactualbehaviorcanbeverycomplicatedasitdependsontherealstructurefactorsandimperfectionsinthematerial. 3 5.5Conclusions WehaveinvestigatedthetemperaturedependenceofthecoerciveeldofMDNinanoparticlesinAl2O3matrix.HcdecreaseslinearlywiththeT2=3.Thisbehaviorcanbeunderstoodaccordingtothestrongdomainwallpinning.Weshowthatthegeneralenergy 66
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barrierthatarisesduetostrongdomainwallpinningdependsonthemagneticeldwithapowerof3/2andisresponsibleforthetemperaturedependenceoftheHc. 67
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CHAPTER6COERCIVEFIELDOFFETHINFILMSASTHEFUNCTIONOFTEMPERATUREANDFILMTHICKNESS:EVIDENCEOFNEELDISPERSEFIELDTHEORYOFMAGNETICDOMAINS 6.1Abstract ThetemperaturedependenceofthecoerciveeldofFethinlmshasbeeninvestigated.Threedierentsamplesofdierentthicknessarestudied.Thecoerciveelddecreaseswithtemperatureandfollowsthesametemperaturedependenceastherstorderanisotropyconstant.ThisbehaviorisconsistentwiththetheoreticalpredictionmadebyNeel 15 basedonthedisperseeldtheoryofmagneticdomainwhichtakesintoaccounttheeectoffreepolesonthecoerciveeldthatoccursatsmallinclusions.Thevalueofcoerciveeldincreaseswithdecreasinglmthickness.Thisbehaviorisexpectedformultidomainferromagneticsystemsatnanoscalewherethedomainwallthicknessiscomparabletoorlargerthanthelmthickness. 6.2Introduction Themostinterestingaspectofferromagnetismisthehysteresisloop, 90 whichreferstothehistorydependentbehaviorofmagnetizationwithappliedmagneticeld(Fig. 62 ).Hysteresisisacomplexnonlinear,nonequilibriumandnonlocalphenomenon,reectingtheexistenceofanisotropyrelatedmetastableenergyminimaseparatedbyelddependentenergybarriers. 3 Anextrinsicpropertyofcrucialimportanceinpermanentmagnetismisthecoerciveeld,themagneticeldwheremagnetizationchangessignasitpassesthroughzero.Thecoerciveeldbasicallydescribesthestabilityoftheremnantstateandisaveryimportantconceptformostpracticalapplications. 91 { 99 Coercivityinferromagnetsisknownfromverylongtime. 90 But,duetothecomplexnature,theoriginofcoerciveeldisstillasubjectofstudy.Inthispresentworkthebehaviorofcoerciveeldofthreedierentironthinlmswithdierentthicknesseshasbeeninvestigated.Thetemperaturedependenceofthecoerciveeldagreeswellwiththetheoryofdomainwallpinningarising 68
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fromsmallinclusions(forexampleimpurityorvacancydefects)wheretheenergyofthefreepoleisnotnegligible. 15 6.3ExperimentalDetails Figure61. TEMimageofFethinlmofthickness9nm. ThinlmsofFewerefabricatedonSi(100)andsapphire(caxis)substratesusingpulsedlaserdepositionfromaluminaandirontargets.HighpuritytargetsofFe(99.99%)andAl2O3(99.99%)werealternatelyablatedfordeposition.Beforedeposition,thesubstrateswereultrasonicallydegreasedandcleanedinacetoneandmethanoleachfor10minandthenetchedina49%hydrouoricacid(HF)solutiontoremovethesurfacesilicondioxidelayer(fortheSisubstratesonly),thusforminghydrogenterminatedsurfaces. 35 Thebasepressureforallthedepositionswasoftheorderof10)]TJ /F3 7.97 Tf 6.59 0 Td[(7Torr.Aftersubstrateheating,thepressureincreasedtothe10)]TJ /F3 7.97 Tf 6.59 0 Td[(6Torrrange.Thesubstratetemperaturewaskeptatabout550oCduringgrowthoftheAl2O3andFelayers.Therepetitionrateofthelaserbeamwas10Hzandenergydensityusedwas2Jcm)]TJ /F3 7.97 Tf 6.58 0 Td[(2overaspotsize4mm1.5mm.A40nmthickbuerlayerofAl2O3wasdepositedinitiallyontheSiorsapphiresubstratebeforethesequentialgrowthofFeandAl2O3.Thisprocedureresultsinavery 69
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smoothsubstrateindependentstartingsurfaceforthegrowthofFe,asveriedbyhighresolutionscanningtransmissionelectronmicroscopystudies(Fig. 21 ).A40nmthickcaplayerofAl2O3wasdepositedtoprotecttheFelayerfromoxidation.Threedierentsampleswiththicknessof9nm,21nmand30nmwerepreparedforthepresentstudy.MagnetizationmeasurementsareperformedinaquantumdesignMagneticPropertyMeasurementSystem(MPMS).Themagneticeldwasalongtheplaneofthelms.Thedependenceoftemperatureandlmthicknessoncoerciveeldisinvestigated. 6.4ResultsandDiscussion Figure62. MHloopofFelmofthickness21nmatdierenttemperaturesasindicatedinthelegend.ThecoerciveelddenedatM=0,decreaseswithincreasingtemperature. ShowninFig. 61 istheTEMimageofthe9nmthickFesample.DuetothelowsurfaceenergydierencebetweenFeandAl2O3(650mJ/m2)andhighadhesionenergy(1205mJ/m2)betweenFeandAl2O3, 100 FewetsthesurfaceofAl2O3andthusacontinuousthinlmisgrowninsteadofgrainsasisthecasefortheNi/Al2O3systemdiscussedinchapter 2 and 3 .Threedierentsampleswiththickness9nm,21nmand30nmweregrown.Themagnetichysteresisloopsatdierenttemperaturesfrom10Kto350Karemeasuredwiththeappliedmagneticeldalongtheplaneofthethinlm.MHloopsfor21nmsampleareshowninFig. 62 .Themagneticeldissweptfrom5 70
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Tto5Tandagainfrom5Tto5Ttocompletetheloop.AthighmagneticeldsthemagnetizationfromtheFesaturatesandthemagneticelddependencearisesduetothediamagneticcontributionfromthesubstrate.ThediamagneticcontributionfromtheFelmisnegligibleasthethicknessofthelmisverysmallcomparedtothethicknessofthesubstrate.Thusthehighmagneticelddataislinearinmagneticeldwithanegativeslope.TheslopeofthelineisdeterminedfromthelineartofthehighelddataandsubtractedfromtherawdatatoextracttheferromagneticsignalduetotheFethinlm.Theprocedureisrepeatedforallsamplesandforalltemperatures.Thecoerciveeldisfoundtodecreasewithincreasingtemperatures.TheresultsforallthreesamplesarepresentedinFig. 63 .Figure 64 showstherelationbetweenK(T) 87 andHc(T)whereTistheimplicitvariable. 87 ThelinearbehaviorofHcandKsuggestthatthecoercivitymechanismissimilartothedisperseeldtheoryofmagneticdomainwhichtakesintoaccounttheeectoffreepolesonthecoerciveeldthatoccursatsmallinclusions. 15 Figure63. Hcvs.TofFelmsofthickness9nm,21nmand30nm.Thetemperaturedependenceofallthreesamplesissimilar,whichsuggeststhattheoriginofthecoerciveelddependsontheintrinsicpropertyoftheiron,whichinourcaseisthemagnetocrystallineanisotropy.Thisistrueasforthecaseofextrinsicorigintheenergybarrierdependsonthesizeofthesampleasdiscussedinchapter 5 71
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Figure64. Hcvs.KofFelmofthickness9nm.ThelinearbehaviorsuggeststhevalidationofNeel'sdisperseeldtheoryofmagneticdomainswhichtakesintoaccounttheeectoffreepolesonthecoerciveeldthatoccursatsmallinclusions(Eq. 6{3 ).Thesimilarbehaviorisobservedforothertwosampleswhichisexpectedastheyhavesimilartemperaturedependence. Theoriesconcernedwiththecoercivityofthemultidomainferromagneticmaterialsbeginwiththeconsiderationofthechangeinmagneticenergyacrossadomainwall. 2 SincethemagnetizationchangesfromMsto)]TJ /F6 11.955 Tf 9.3 0 Td[(Msacrossa180odomainwall,theeectivepressureonthewallwillbethedierenceintheenergyacrossthewallperunitvolume.AtanappliedmagneticeldH,thepressurewillbe2HMs.Thustheworkdonetomoveadomainwallofareastoadistancedxwillbe 2 dW=2HMssdx(6{1) Theaboveequationcanbegeneralizedforanyangle(notonly180o)domainwall. 2 ThetermdW=dx,whichisbasicallytheenergyrequiredtomoveadomainwalltounitdistance,isthemeasureoftheresistanceofdomainwallmotion. 2 Inrealsamplesduetoimpurities,imperfectionsorirregularitiesincrystal,dW=dxpassesthroughmaximumandminimum.Theoriginofreversibilityinthemagnetizationloopistheirreversiblemotionofdomainsthroughthesemaximumandminimum. 2 Thecoerciveeldisusuallycalculatedusingtheequationbelow. 2 72
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Hc=1 2Mss(dW=dx)max(6{2) Dierenttheoreticalapproachesconcentrateonthederivationof(dW=dx)max.SubstantialwallmotionmayrequireeldsoftensorhundredsofOersted.Evidentlyrealmaterialscontaincrystalimperfectionsofonesortoranotherwhichhindertheeasymotionofdomainwalls.Thesehindrancesaregenerallyoftwokinds:inclusionsandresidualmicrostress. 2 Fromamagneticpointofview,an"inclusion"inadomainisaregionwhichhasadierentspontaneousmagnetizationfromthesurroundingmaterial,ornomagnetizationatall.AccordingtotheresultobtainbyNeelinhisdisperseeldtheory(whichbasicallycalculatestheterm(dW=dx)max),coercivityisgivenbyEq. 6{3 below. 15 Hc=1 4v122 KMs+Kv2 Ms(6{3) Thersttermisduetotheresidualmicrostressandv1isthevolumefractionofthefreepoleattheresidualmicrostressand;;KandMsarethesaturationmagnetostriction,internalstress,magnetocrystallineanisotropyconstantandsaturationmagnetizationrespectively.ThesecondterminEq. 6{4 originatesduetothepolesattheinclusionsofvolumefractionv2.Foriron,Ms=1743emu/cm3, 2 K=8x106ergs/cm3, 101 =10x10)]TJ /F3 7.97 Tf 6.58 0 Td[(6 102 and=1010dynes/cm2. 103 PuttingthesevaluesintheEq. 6{3 weobtain, Hc'0:18v1+4600v2Oe(6{4) Thusinourcasethecoerciveeldwillbedominatedbythe2ndterminEq. 6{3 ,whichisproportionaltoKandagreeswellwiththeexperimentalresultsasshowninFig. 63 andFig. 64 .RememberthatMsisconstant. InFig. 65 thevariationofHc(d)isshown.TheincreaseinHcwithdecreasinglmthickness,d,couldbeduetotheenhancementofKwithdecreasingd. 101 104 105 Theincreaseincoerciveeldwithdecreasingthicknessiswellknownforthemultidomain 73
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Figure65. Hcvs.dofFelmsat10K.Coerciveeldincreaseswithdecreasingd.ThisbehaviorisduetofactthatKincreaseswithdecreasingdwhichisverycommoninmultidomainthinlmswhenthedomainwallthicknessiscomparableorlargerthanthelmthickness.Thedomainwallthicknessofironisabout60nm, 3 whichislargerthanthethicknessofthelmsstudiedhere. magneticthinlmswhenthedomainwallthicknessiscomparabletoorhigherthanthelmthickness. 76 Thedomainwallthicknessofironisabout60nm, 3 whichislargerthanthethicknessofthelmstudiedhere.NotethatwehaveusedthevalueofKinEq. 6{3 ,whichislargerthanthebulkvalue.FromEq. 6{4 ,wendthatv20:12. 6.5Conclusion ThecoerciveeldofmultidomainFethinlmshasbeeninvestigated.ThetemperatureandthicknessdependenceofthecoerciveeldagreeswellwiththepredictionmadebyNeel,whichtakesintoaccounttheeectoffreepolesonthecoerciveeldthatoccursatthesmallinclusions.ThecontributionofstraintothecoercivityisverysmallforthecaseofFeandthedominantcontributioncomesfromthefreepolesattheinclusions.Thevolumefractionofinclusionshasbeenestimatedfromthecoerciveelddatatobearound0.12. 74
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CHAPTER7SCALINGCOLLAPSEOFTHEIRREVERSIBLEMAGNETIZATIONOFFERROMAGNETICTHINFILMS 7.1Abstract Inferromagneticmaterials,hysteresis,orequivalentlythehistorydependentbehaviorofthemagnetization,reectscomplexnonlinearandnonequilibriumphenomenologythathasbeenrecognizedformanyyears 5 6 106 { 108 .Hysteresisdependsstronglyonmaterialspropertiessuchasstructurallengthscalesspanningthenanometertomicrometerrange 3 andmanifestscomplexbehaviorsincludingmagneticrelaxationwithagingdependence 109 ,dimensionallydependentdipoledipoleinteractions 48 110 ,spinglasslikememoryeects 111 andsupermagnetism 112 .Hereweshowthattheirreversiblemagnetization,denedasthedierencebetweeneldcooledandzeroeldcooledmagnetization,hasastrikingsimilarityforawidevarietyofferromagneticmaterials.Thissimilaritybecomesapparentwhentheirreversiblemagnetizationisnormalizedtoitsmaximumvalueandplottedwithrespecttoatemperaturedependentrenormalizedeld.Thecollapseoftheirreversiblemagnetizationontoasinglecurveforagivensystemimpliesanunderlyingsymmetrytohysteresisthatisnotcapturedbypreviousanalytical 3 5 6 48 106 107 109 { 112 andcomputationaltreatments 108 113 andthusprovidesaunifyingthemethatembracesabroadrangeofcomplexhystereticbehavior. 7.2Introduction Ingeneral,hysteresisisacomplexnonlinearnonequilibriumphenomenonwhichreectsthepresenceofelddependentenergybarriersbetweenanisotropydependentmetastableminima.Accordingly,hysteresisisaectedbyacombinationofintrinsicpropertiessuchasmagnetocrystallineanisotropywhichdependsoncrystaleldenergyandspinorbitcouplingandextrinsicpropertiessuchassampleshape,grainboundaries,disorderandimperfections.Forexample,inbulkferromagnetshysteresisisoftendescribedasasuperimpositionofdomainwallmotionanddomainrotationwithenergybarriersrelatedtomagnetocrystallineanisotropytogetherwithimperfections 75
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and/orimpuritiesinthematerial 107 .Forthesimplestcaseofsingledomaincoherentlyrotatingnanoparticles,theoriginofhysteresisisthenitetimescaleformagnetizationreversalasthemagnetizationovercomesamagneticelddependentenergybarrierbythermalactivationandrotatesfromoneeasyaxisdirectiontoanother 5 6 106 .Hysteresisandassociatedmagnetizationreversalsplayanimportantroleinapplicationssuchasmagneticdatastoragedevices 91 { 93 ,GMR 94 95 orMRAM 96 devices,magneticsensors 97 andmotors 98 ,generators 99 etc. 7.3ExperimentalResults Measurementsofirreversiblemagnetizationareusuallyaccomplishedbyoneorbothoftwotechniquesillustratedrespectivelyinpanelsa)andb)ofFig. 71 .Thesampleunderinvestigationinthisgure(hereafterreferredtoasampleA)isa20Athickpulsedlaserdepositedthinlmcomprisingvelayersof3nmelongatedNiparticlesembeddedinaninsulatingAl2O3host[seeMethods].TheNiparticlesaresmallenoughtobeinthesingledomain(SD)regimewhereallthespinsarealignedinthesamedirectionandrotatecoherentlytogetherinresponsetoachangingmagneticeld.Inthersttechnique(panela),thesampleiseldcooled(FC)inaeldH=20Oe(blacksquares)from300Kto5Kandthenzeroeldcooled(ZFC).Theirreversiblemagnetization(M(H;T)),whichisafunctionofmagneticeld(H)andtemperature(T),isshownbythetwoheadeddashedverticalarrow.Inthesecondtechnique,thesampleisheldatxedtemperatureTandmagnetizationMloopsobtainedbyrepeatedlycyclingtheappliedeldHaboutH=0betweentwosymmetriclimits.Thehistorydependenttrajectoriesformclosedloopsshownschematicallyintheinsetsofpanel(b).Theseloops,whichcanbeacquiredatdierenttemperatures,areeachcharacterizedbyacoerciveeldHc(T),asaturatedmomentMs(T)andaremnantmagnetizationMr(T).ThecoerciveeldHc(T),plottedversusT1=2inpanelbforsampleAdiscussedabove,isshownasabluelineconnectingthestarreddatapoints.TheabsenceofaT1=2dependenceforcoherentlyrotatingSDparticleswitheasyaxesorientedalongtheeld 6 willbediscussedbelow.WhilebothM(H;T)andHc(T) 76
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Figure71. IrreversiblemagnetizationM(H;T)denedasthedierenceoftheFCandZFCmagnetizationsisaquantitativemeasureofhysteresis.a,BlacksquaresandredcirclesrepresentrespectivelytheFCandZFCtemperaturedependentmagnetizationsforsampleAina20Oeeldappliedparalleltothelmsurface.TheirreversiblemagnetizationM(H;T)isshownbythetwoheadedverticaldottedarrow.Inset:Largethermallyblockedmagneticparticles(1and3)withrespectiveverticalandhorizontaleasyaxesofmagnetizationindicatedbythearrows.Particle2issmallenoughtobesuperparamagnetic(thermallyunblocked).Formagneticeldsappliedalongtheverticaldirection,particles2and3donotcontributetoM(H;T).b,Thecoerciveeld(Hc)forthesamesampleshownasafunctionofT1=2(Bluestars)doesnotshowthelinearbehaviorexpectedforidealStonerWohlfarthparticles 6 wherealltheparticlesareuniformsizeandalignedwiththeappliedeld(particle1).Thesolidbluelineisattothedatausingalognormaldistributionofparticlesizetogetherwitharandomorientationoftheeasyaxisofthemagnetizations.Inset:Schematicmagnetizationcurvesforthecaseswhere(b1)onlyparticles1and2and(b1)onlyparticles1and3arepresent.Theresultantmagnetizationloops(blackcurves)forthetwocasesshowthepronouncedeectsofparticlesizeandeasyaxisorientationonthedeterminationofHc. arecommonlyacceptedmeasuresofhysteresis,theunderlyingphenomenologyforeachisconsiderablydierent.ForexampleinnanoparticlemagneticsystemssuchasshowninFig. 71 ,M(H;T)andHc(T)aresensitiveindierentwaystoboththepresenceofsuperparamagneticparticlesandtherandomorientationoftheeasyaxisofmagnetizationofeachparticle.TheinsetsofFig. 71 a)andb)schematicallyillustratethesedierencesusingthreeparticles:particles1(red)and3(blue)witheasyaxesofmagnetization 77
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respectivelyalongthevertical(H)andperpendiculardirectionsandlargeenoughsothatatthetemperatureofmeasurement,changesinmagnetizationareblockedbyenergybarriersthatcannotbeovercomebythermalactivation,andparticle2(green)witheasyaxisalongtheverticalaxisandsmallenoughsothatitissuperparamagneticwithanonhystereticmagnetizationdependingonlyonHandT(i.e.,unblocked).Considerthecasewhereonlyparticles1and2arepresent.Sincethesuperparamagneticparticle2willhavezeroM(H;T),thetotalM(H;T)valuewillbeonlyduetotheblockedparticle1.Ontheotherhand,theMHloopwillbethesummedcontributionsofthehystereticloopforparticle1andthereversibleloopforparticle2asshownininsetb1ofFig. 71 b.ThusforthiscaseM(H;T)isnotaectedbysuperparamagneticparticlesbutHc(T)is.Considernowthecasewhereonlyparticles1and3arepresent,i.e.,bothparticlesareblockedbutwithdierent(parallelandperpendicular)easyaxisorientationswithrespecttotheappliedeld.SimpletheoryforcoherentlyrotatingSDparticlesshowsthatuponreversingtheeldparticle1mustsurmountaHdependentenergybarrierwhereasparticle3canlineupwithouthavingtoovercomeanenergybarrier 3 .Inlikemannertothepreviouscase,TheMHloopforparticle1showshysteresisbutparticle3doesnot(insetb2ofFig. 71 b).HenceHc(T)isaectedbythepresenceofparticleswithperpendicularorientationbutM(H;T)isnot. TheaboveargumentscanbegeneralizedforSDmagneticnanoparticleswithabroadsizedistributionandarandomorientationoftheeasyaxesofmagnetization.Particleswithaneasyaxismakinganarbitraryanglewiththeappliedmagneticeldwillalwayscontributelesstohysteresisthanalignedparticles.Becausetheperpendicularcomponentdoesnotcontribute,thecorrectionisastraightforwardintegrationoverangle 7 .Accordingly.themeasuredvalueofM(H;T)willbeonlyduetoblockedparticlesanddominatedbyparticleswitheasyaxisofthemagnetizationalongtheappliedmagneticeld.Ontheotherhand,Hc(T)willbestronglyaectedbytherandomorientationoftheeasyaxisofblockedparticlesandthepresenceoftheparticleswhicharesmallenoughto 78
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besuperparamagnetic.ForanidealStonerWohlfarthparticlesystem 6 inwhichalltheparticlesarealignedalongtheHdirection,alinearsquareroottemperaturedependenceofHc(T)isexpected.FortheconsiderablymorecomplicatedcaseofrandomlyorientedSDparticleswithasizedistributioninwhichsomeoftheparticlesaresuperparamagnetic(e.g.,sampleA),Hc(T)canbedescribed(solidlineofFig. 71 b)usingamodelwithalognormalsizedistributionandthreettingparameters 9 10 (seeMethods).TheHdependentbehaviorofM(H;T)forsampleAisshowninFig. 72 aforthetemperaturesindicatedinthelegend.Theisothermsshowpeaks,Mmax(T),atmagneticelds,Hm(T),indicatedbytheverticalarrows.Thesepeaksareexpected,sinceatH=0theFCandZFCmeasurementsareequivalentandthedierenceinmagnetizationshouldbezero,whereasathighHbothFCandZFCmagnetizationssaturatetothesamevalueandagainthedierenceshouldgotozero.ThesimilaritiesintheM(H;T)isothermsaresuggestiveandbecomemanifestasanunexpecteddatacollapseontoasinglecurvewhenthereducedirreversiblemagnetization,M(H;T)=Mmax(T),isplottedasafunctionofreducedmagneticeld,h(T)=H=Hm(T),asdoneinFig. 72 b.ThecharacteristiceldHm(T)deviatessignicantlybelowHc(T)forT<25K(insetofFig. 72 b)andidentiestheTdependenteldwhereirreversibilityisatamaximum. AnimportantphysicalinsightintothescalingcollapseshowninFig. 72 bisgainedbyplottingMmax(T)asafunctionofT1=2.TheobservedlinearbehaviorshowninFig. 73 aisidenticaltothepredictedtemperaturedependentcoercivityHSWc(T)ofStonerWohlfarth(SW)particles 6 mentionedabove.Guidedbythissimilarity,wemaketheansatz:Mmax(T)/HSWc.Thisansatzisphysicallyreasonablesinceasshownabove,M(H;T)measurementsarenoteectedbythepresenceofsuperparamagneticparticles,andinadditionthecontributionfromparticleswitheasyaxisofmagnetizationalongthemagneticeldisdominant.Asallrealsamplescompriseparticlesizedistributionsandrandomeasyaxisorientations,theconventionalMHloopsfromwhichcoercivitiesareextractedaremarkedlydierentthanwouldoccurforidealized 79
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Figure72. AllofthedataforM(T;H)ofsampleAcan,withpropernormalization,bemadetocollapseontoasinglecurve.a,IsothermsofMplottedasafunctionofHshowselfsimilarbehaviorwithmaximaMmax(T)occurringatcharacteristiceldsHm(T)markedbytheverticalarrows.WithdecreasingtemperatureMmax(T)increasesandHm(T)movestohigherelds.b,ThescalingcollapseoccurswhenM(H;T)=Mmax(T)isplottedagainstthenormalizedeldH=Hm(T).Inset:PlotsofHm(squares)andHc(T)(stars)asafunctionofT.ThedataandtforHcarethesameasshowninFig.1b,butplottedwithrespecttoTratherthanT1=2.ThesolidlineforHm(T)isaguidetotheeye. SWbehavior.TheinsensitivityofM(H;T)measurementstosuperparamagneticparticlesandperpendicularorientationsofblockedparticlestogetherwithouransatzimplythatmoreusefulinformationaboutthemagnetizationreversalprocessisobtainedfromM(H;T)measurementsthanHc(T)measurements. 80
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Figure73. ForsingledomainparticlestheansatzMmax(T)/HSWcisveried.a,ThelineardependenceofMmax(T)onT1=2isinaccordancewiththeStonerWohlfarththeoreticalpredictionthatHc(T)/T1=2forthecoherentlyrotatingsingledomainparticlesofsampleA.TheuseofMmax(T)ratherthanHc(T)asameasureofhysteresisremovestheeectsofnonuniformparticlesizeandrandomorientation.b,ThevaluesofHcalc(T),computedforuniformsizeFePtparticles(sampleB)fromtheansatzderivedEq.2attheindicatedtemperatures,scalelinearlywithHSWc(T)whichisdeterminedfromthecoerciveeldsofM)]TJ /F6 11.955 Tf 11.95 0 Td[(Hloopsaftercorrectionfortherandomorientationoftheeasyaxisofmagnetization(seeMethods). ThescalingcollapsebehaviorplottedforsampleAinFig. 72 bsuggeststhatMhastheform, M(H;T)=Mmax(T)F(H=Hm(T));(7{1) whereFisanunknownfunctionwiththepropertyF(1)=1.TakingthesecondpartialderivativeofthebothsidesofthisequationandsolvingforMmax(T)givestheresult:Mmax(T)=(@2F(h)=@h2))]TJ /F3 7.97 Tf 6.59 0 Td[(1h=1H2m(T)@2M(H;T)=@H2Hm(T),evaluatedatthe 81
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maximumwhereh(T)=H=Hm(T)=1.Therstterm,(@2F(h)=@h2))]TJ /F3 7.97 Tf 6.58 0 Td[(1h=1,mustbeaconstantbecauseofthescalingcollapse.Theremainingtwotermshavethesameformastheexpectedvalueofaneectiveanisotropyeld 114 .Thusaccordingtoouransatz,Mmax(T)/HSWc,wecanwritetherelation HSWc(T)=CH2m(T)@2M(H;T)=@H2Hm(T)=CHcalc(T);(7{2) whereCisaconstantandHcalc(T)=H2m(T)@2M(H;T)=@H2Hm(T)iscomputedfromexperimentaldata. TotesttheresultexpressedinEq.2,weusemagnetizationdataonasystemofuniformsize(6nmdiameter)FePtnanoparticles(sampleB,seeMethods)synthesizedviathermaldecompositionofFe(CO)5andreductionofPt(acac)2 115 .ThemeasuredcoerciveeldHMHc(T)isobtainedfromMHloopsatdierenttemperatures.Assumingthattheparticleseasyaxesofmagnetizationarerandomlyoriented,atemperaturedependentcorrectiontoHMHc(T)mustbemadesothatHSWc(T)canbeinferred.Thiscorrectionisneeded(seeMethods)sincethemagnetizationofrandomlyorienteduniformsizeparticlesshowsaT3=4dependence 7 comparedtotheT1=2dependenceexpectedforanidealizedsampleinwhichalltheparticlesarealignedalongtheappliedmagneticeld.TheplotofFig. 73 includesthiscorrectionandshowsalineardependenceofHcalc(T)onHMHc(T)aswouldbeexpectedforasystemofcoherentlyrotatingSDuniformsizeFePtnanoparticles.Thelinearbehaviorwithslopeof1.09(4)conrmsthevalidityofourmodelasexpressedbyEq.2withC1.InFig. 74 thereducedirreversiblemagnetization,M(H;T)=Mmax(T),isplottedasafunctionofreducedmagneticeld,h(T)=H=Hm(T)forawidevarietyofthinlmmagneticmaterialslabeledintheinsetanddescribedinMethods.Unexpectedly,whenplottedinthismanner,themagnetizationdataforeachmaterialssystemcollapseontosinglecurveswhichhavesimilarshapesdescribedbyauniquefunctionF(H=Hm(T))(seeEq.1)foreachsystem.Thisdatacollapseisquiteremarkableconsideringthevarietyofmechanismsresponsible 82
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Figure74. Scalingcollapsedescribesirreversiblemagnetization(hysteresis)inawidevarietyofferromagneticmaterials.a,PlotsofthereducedirreversiblemagnetizationM(H;T)=Mmax(T)asafunctionofreducedmagneticeldH=Hm(T)forthesixdierentmagneticmaterialslabelingeachcurve.TheimplicittemperaturevariableincreasesfromlefttorightandeachcoloronagivencurverepresentsadierentM(H;T)isotherm.Forclarity,theordinatevalueshavebeenshiftedandthesolidlineshavebeenaddedasguidestotheeye.ThebottommostcurveforsinglecrystalspinglassCu:Mn(at.1.5%)materialistakenfromtheliterature 116 formagneticorderingtogetherwithawiderangeofmaterialsproperties.Thescalingcollapseappliesequallywell:tosingledomain(SD)coherentlyrotatingNinanoparticleswithaverageparticlediameterof3nmembeddedinaninsulatingmatrix;tomultidomain(MD)incoherentlyrotatingNinanoparticleswithaverageparticlediameterof12nmalsoembeddedinaninsulatingmatrix;tocoherentlyrotatinguniformsizeFePtnanoparticles(6nmdiameter);tocontinuousmetallicGdthinlmswithmagnetizationderivedfromlocalmomentssupplementedbybandstructureexhibitingsomeitinerantcharacter;andtomixedphasemanganite(LPCMO)wheretheMnspinsorderbyadoubleexchangemechanisminanenvironmentwherechargeorderedandparamagneticinsulatingphasescompetewithaferromagneticmetallicphase.Wehavealsoincludedaspinglassmaterial,singlecrystalCu:Mn(1.5at%),describedintheliterature 116 .ThecollapseoccursfornanoparticlesystemswhichincludeSD,MDandsuperparamagneticparticleswithboth 83
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broadanduniformsizedistributionsandmagneticmomentreorientationsarisingfromcomplexsuperimpositionsofdomainwallmotionanddomainrotationwhichcanbeverydierentincontinuouslmscomparedtonanoparticleswheretheextentofthedomainwalliscomparabletothesizeoftheparticle.Thusthematerialsmeasuredhereareverymuchdierentintermsoftheoriginoftheirreversiblemagnetization. Inconclusion,wehavepresentedaheretoforeunreportedphenomenologicalresultshowingthatthetemperatureandelddependenthysteresisofatleastsixdistinctlydierentmagneticsystemscanbecollapsedontosinglecurves(Fig. 74 )usingtheparticularlysimplefunctionalformexpressedbyEq.1.Ourndingthatsuchascalingcollapseappliestomagneticsystemstotallydierentthanthespinglassforwhichsimilarscalinghasbeenpreviouslynoted 116 117 (thelowestcurveinFig. 74 )suggeststhatexplanations 116 relyingonspinglassphenomenologyaretoonarrow.Thusamoregeneraltheoryisneededtoexplainthescalingcollapse.Thiscollapsemustimplyanunderlyingsymmetrythatisnotcapturedbypreviousanalyticalandcomputationaltreatmentsandmaybeacrucialcluetounderstandthecomplexhistorydependentmagnetizationprocess.ThesimilaritywiththespinglassmaterialisinterestingandmaybebecauseofthefactthatallZFCmagnetizationisametastablestateofthesystemandshowspropertiesvaryingwithtime.Thusthedynamicsofthespinsmayplayaveryimportantroleforthescalingcollapse.ThebehaviorofMmax(T)isinvestigatedforthe3nmNiparticles.WesuggestanewapproachtoinvestigatethemagnetizationreversalprocessfromtheMmax(T)measurement.WehavesuccessfullyappliedthemethodforthecoherentlyrotatingSDparticles. 7.4Conclusions Inconclusion,wehavepresentedasurprisinglygeneralandunrecognizedphenomenologicalresultshowingthatthetemperatureandelddependenthysteresisofatleastsixdistinctlydierentmagneticsystemscanbecollapsedontosinglecurves(Fig. 74 )usingtheparticularlysimplefunctionalformexpressedbyEq.1.Wehavenotyetfound 84
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anyexceptions.Fortheparticularlysimplecaseofcoherentlyrotatingsingledomainparticles(samplesAandB),ouranalysisofscalingcollapsebypassesthecomplicationsofnonuniformsizedistributionsandrandomeasyaxisorientation,unveilinganunderlyingStonerWohlfarthbehavior 6 .Ourndingthatthesamescalingcollapsemoregenerallyappliestomagneticsystemswithawidevarietyofmechanismsgivingrisetohysteresis,suggeststhatexplanations 116 relyingonspinglassphenomenologyaretoonarrow.Thusamoregeneraltheoryisneededtoexplainthescalingcollapse.Thiscollapsemustimplyanunderlyingsymmetrythatisnotcapturedbypreviousanalyticalandcomputationaltreatmentsandmaybeacrucialcluetounderstandcomplexhistorydependentmagnetizationprocesses.Thesimilaritywiththespinglassmaterial 116 issuggestiveandmayberelatedtothefactthatallZFCmagnetizationsrepresentmetastablestatesofthesystem,whichifgivensucienttimewouldrelaxtowardtheeldcooledequilibriumstate.Accordingly,thedynamicsofthespinsmayplayaveryimportantroleinunderstandingthescalingcollapse. 7.5Methods 7.5.1NiNanoparticle. CompositelmscomprisingmagneticNinanoparticlesembeddedinanAl2O3hostmatrixweresynthesizedbypulsedlaserdeposition(PLD) 36 .HighpuritytargetsofNi(99.99%)andAl2O3(99.99%)werealternatelyablatedinthesamedepositionrun.Thebasepressureofthedepositionwasontheorderof10)]TJ /F3 7.97 Tf 6.58 0 Td[(7Torr.Thesubstratetemperaturewasmaintainednear550Cduringthegrowth.Therepetitionrateofthelaserbeamwas10Hzandenergydensityusedwas2Jcm)]TJ /F3 7.97 Tf 6.58 0 Td[(2overaspotsizeof4mm1.5mm.A40nmthickbuerlayerofAl2O3wasdepositedinitiallyonthesapphiresubstratebeforethesequentialgrowthofNiandAl2O3.ThisprocedureresultsinaverysmoothstartingsurfaceofgrowthofNiasveriedbythehighresolutionscanningtransmissionelectronmicroscopy(STEM)studies.Samplesconsistsof5layersofNiandAl2O3.AcaplayerofAl2O3wasalwaysusedtoprotectthesamplefromoxidation.ZcontrastSTEMimage 85
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veriestheabsenceoftheNioxide.SamplesstudiedhereconsistsofNiparticlesizeof3nmand12nmindiameter. 7.5.2GdThinFilm. GdthinlmsweredepositedonSisubstratesbyDCmagnetronsputtering.Thebasepressureofthechamberwasontheorderof510)]TJ /F3 7.97 Tf 6.59 0 Td[(7Torr.Thesamplesarecontinuouswiththicknessnear100nm. 7.5.3(La1)]TJ /F5 7.97 Tf 6.59 0 Td[(yPry)0:67Ca0:33MnO3(LPCMO)ThinFilms. Phaseseparatedmanganite(La1)]TJ /F5 7.97 Tf 6.59 0 Td[(yPry)0:67Ca0:33MnO3(LPCMO)lmsweregrownusingpulsedlaserdeposition(PLD)atarateof0.05nm/sonNdGaO3(NGO)(110)substrateskeptat820Cinanoxygenatmosphereof420mTorr 118 7.5.4TemperatureCorrectionofCoerciveField. ForidealStonerWohlfarthparticlesthecoerciveeldisgivenby,HSWc=Hco(T)(1)]TJ /F1 11.955 Tf 453.9 23.9 Td[((T=TB)1=2).Forthecaseofrandomlyorientedcoherentlyrotatingparticlesallofwhichhavethesamesize,thecoerciveeldisgivenby,Hranc(T)=0:48Hco(T)(1)]TJ /F1 11.955 Tf 12.36 0 Td[((T=TB)3=4).SincetheFePtparticlesofsampleBallhavethesamesize,wecanwriteHranc(T)=HMHc(T)whereHMHc(T)isthecoerciveeldextractedfromthemagnetizationloops.Itisthenstraightforwardtoshowthat,HSWc(T)=2HMHc(T)(1)]TJ /F1 11.955 Tf 12.13 0 Td[((T=TB)1=2)=(1)]TJ /F1 11.955 Tf 12.13 0 Td[((T=TB)3=4).Usingthefactthatatloweldsthezeroeldcooledpeaktemperaturecanbeidentiedastheblockingtemperature 119 ,wendthatTB=60KfortheFePtnanoparticles.AccordinglyHSWc(T),theabscissainFig. 73 b,canbecalculatedinastraightforwardmannerfromthemeasuredvaluesofTBandHMHc(T). 86
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BIOGRAPHICALSKETCH RiteshKumarDaswasbornon1981inaverysmallvillage,Mohanbati,locatedeastofIndia.AtHaripalGuruDayalhighschool,Riteshwasintroducedtophysicsandfellinlovewiththesubject.Riteshgotinterestedinsciencesubjectsduringhishighschooldays,wherehefoundwonderfulteachers,Mr.RobinChatterjeeandMr.UttamSaha.Aftercompletingthehighschool,RiteshenrolledintheRamakrishnaMissionVidyamandira(Belur)inAugust1999andgraduatedwithaBachelorofSciencedegreewithhonorsinphysicsonAugust2002.DuringthistimeRiteshmethisfavoriteteacherDr.DeepakGhsosh,whoplayedaverycrucialroletomakeRiteshinterestedinexperimentalphysics.AftercompletingtheBachelorofSciencedegree,RiteshenrolledinMasterofSciencedegreeatIndianInstituteofTechnology(Kanpur)andcompletedthedegreeonAugust2004.AfterthisRiteshjoinedUniversityofFloridatopursuehisPh.D.degree.RiteshwasalwaysinterestedinthepropertiesofmaterialsatnanoscaleandfoundthatProf.A.F.Hebard'slabtobetheperfectplacefortheresearchintheeldofthinlmsandnanoparticles.RiteshgraduatedinAugust2010withaDoctorofPhilosophydegreeinphysics. 96

