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Universal susceptibility variations in 1 q 1 dimensional vortex glass


Academic year: 2021

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Universal susceptibility variations in 1


1 dimensional

vortex glass

Chen Zeng


, P.L. Leath


, Terence Hwa

b a

Department of Physics and Astronomy, Rutgers UniÕersity, PO Box 849, Piscataway, NJ 08854-0849, USA b

Physics Department, UCSD, La Jolla, CA 92093, USA


Ž .

We model a planar array of fluxlines as a discrete solid-on-solid SOS model with quenched disorder. Simulations at finite temperatures are made possible by a new algorithm that circumvents the slow glassy dynamics encountered by traditional Metropolis Monte Carlo algorithms. Numerical results on magnetic susceptibility variations support analytic predictions.q2000 Elsevier Science B.V. All rights reserved.

Keywords: Flux pinning; Glassy state; Magnetic susceptibility; Disorder

1. Introduction

Over the years, various low-temperature glass phases have been proposed for vortex matter in dirty

w x

type-II superconductors 1 . Understanding the ther-modynamics of such interacting many-body systems in the presence of quenched disorder remains a challenge. Similarities between the randomly pinned vortex system and the more familiar mesoscopic

w x

electronic systems 2 are highlighted by a recent experiment on vortices threaded through a thin

crys-w x

tal of 2H-NbSe by Bolle et al. 3 . Sample-depen-2

dent magnetic responses known as ‘‘magnetic finger prints’’ have been observed for such a mesoscopic vortex system.


Corresponding author. Fax:q1-908-445-4343.

The simplicity of the planar vortex system al-lowed detailed theoretical studies of this glassy

w x

system 4a,4b–9 , with quantitative predictions in-cluding the universal sample-to-sample variation of magnetic responses. However, until the work of Bolle et al., there were hardly any experimental studies of this system, with difficulties stemming partly from the weak magnetic signals in such 2d systems. Meanwhile, progress on numerical ap-proaches was also seriously hampered by the slow glassy dynamics often encountered in simulations at

w x

finite temperatures 10a,10b,10c . To overcome this numerical difficulty, we model a planar array of

Ž .

fluxlines as a discrete solid-on-solid SOS model, viz., a dimer model with quenched disorder. A new polynomial algorithm circumventing the glassy dy-namics enables us to simulate large systems of this discrete model at any finite temperature.

0921-4534r00r$ - see front matterq2000 Elsevier Science B.V. All rights reserved.

Ž .


of a given covering, and T is the dimer temperature.d Quenched disorder is introduced via random bond energies ei j, chosen independently and uniformly in

Ž Ž . Ž ..

the interval y1r2 , 1r2 .

The dimer model is related to the planar vortex-line array via the well-known mapping to the SOS

Ž . 4

model see Fig. 1 : Define integer heights h at the centers of squares of LL, which form the dual square lattice LLD, then orient all bonds of LLD such that

elementary squares of LLD that enclose sites of a

Ž Ž ..

chosen sublattice of LL solid dots in Fig. 1 a are

circled counterclockwise; Assign y3 to the

differ-ence of neighboring heights along the oriented bonds if a dimer is crossed andq1, otherwise. This yields

single-valued heights up to an overall constant. In

Ž .

terms of the height configuration h r , the partition

Ž .

function 1 can be written alternatively as Zs

ÝhŽr.4eybHHwhx, where the SOS Hamiltonian takes the

following form in the continuum limit,

K 2 2 bHHs


d r




yf r

Ž .

P=hqgcos Gh



. 2 2

Ž .

Here, K is an effective stiffness caused by the inability of a tilted surface to take as much advan-tage of the low weight bonds as a flatter surface, and

Ž . Ž .

Fig. 1. a Snapshot of a dimer covering thick bonds together

Ž .

with the associated ‘‘height’’ values h r for a lattice of size

Ž .

Ls8 at temperature Tds1.0. b Dimer covering of the fixed

Ž . Ž .

reference. c Vortex line configuration thick lines obtained as

Ž . Ž .

the difference between a and b .

3. The algorithm

Computing the partition function of complete dimer coverings on a weighted planar lattice GG can

w x

be achieved in polynomial time 11,12a,12b . Weights

here refer to the Boltzmann factors wi j'

Ž .

expyei jrTd on the bonds. In this article, we shall w x

use the shuffling algorithm by Elkies et al. 13a and

w x

Propp 13b to sample the configurational space. The algorithm relates the partition function Z on a lat-L

Ž 4.

tice of linear size L to Z as Z w s

Ly1 L

Ž 4. Ž X4.

C w ZLy1 w after a simple weight

4 X4 Ž 4.

tion w ™ w . The prefactor C w is independent

of dimer coverings. The partition function is ob-tained in a ‘‘deflation’’ process in which the above

recursive procedure is carried out down to Ls0

with Z s1. This deflation process can also be


reversed in an ‘‘inflation’’ process where a dimer covering at size Ly1 can be used to stochastically

generate a dimer covering at size L according to ZL already obtained. Repeating the inflation process, thus, generates uncorrelated ‘‘importance samplings’’ of the dimer configurations, or, equivalently, the equilibrium height configurations, without the need to run the slow relaxational dynamics. The ensuing numerical results are obtained by taking various measurements of the height configurations generated this way. A somewhat inconvenient feature of this approach is that the algorithm requires open bound-ary condition on the dimer model; this in turn fixes the total number of vortex lines, e.g., to Lr2 on a

Ž .

L=L lattice see Fig. 1 .

4. Numerical results

Since the temperature of the vortex array, given y1

Ž .

by K in Eq. 2 , is generally different from the



Ž . Ž .

Fig. 2. a The disorder-averaged thermal displacement fluctuation WT L for various dimer temperatures T . Each data point was obtainedd

3 3 2 y1

Ž . Ž . Ž .

by generating 10 thermal samplings for each of 10 disorder realizations. The straight lines are fit to WTs2pK ln Lqconst. b The extracted relation between Ky1 and T . The horizontal line indicates the asymptotic value of Ky1 as T`.

d d

temperature scale. To do so, we exploit a statistical

w x Ž .

rotational symmetry 9,15 of the system 2 , which guarantees that at large scales, the effective K is the same as that of the pure system. In particular, K can be obtained by measuring the disorder-averaged ther-2

mal fluctuation of the displacement field WT

2 2 Ž .y1 Ž .




Ž .

r % y$ht

Ž .

r %


s 2pK ln L ,

Ž . Ž . ² Ž .:

where h r 'h r y h r measures the thermal


distortion superposed on the distorted ‘‘background’’

² Ž .:h r by the quenched disorder. We used $. . .%, ². . . , and overline to denote spatial, thermal, and:

disorder averages, respectively. With the polynomial algorithm, we were able to perform thorough disor-der averages for equilibrated systems of sizes up to

512=512. To reduce boundary effects, we focus on

the central Lr2=Lr2 piece of the system and

Ž .

compute its displacement fluctuations. Fig. 2 a

illus-2Ž .

trates the dependence of WT L for various dimer

Ž .

temperatures T . The linear dependence on ln L isd

apparent. Identifying the proportionality constant

Ž .y1

with 2pK , we obtain the empirical relation


Ž .

tween K and T shown in Fig. 2 b . Note that ourd


Ž .

result recovers the exact relation K T ™` s


16rp for the dimer model without disorder

w14a,14b . Since the glass transition of the system 2x Ž .

is expected to occur at temperature Ky1



16rp, our system is glassy for the entire range of

dimer temperatures.

To probe this glassy state further, we now focus on its magnetic response, i.e., the uniform magnetic susceptibility x. Due to the constraint of fixed

vor-tex density when using the dimer representation, it is not easy to compute the magnetic susceptibility


rectly by varying the vortex fugacity i.e., external

Ž . 2 Ž . 2

Fig. 3. a q C q vs. q . Different symbols denote different disorder realizations, all of which are for L2 s128 at Tds0.04. The

Ž . Ž . 3

susceptibility x is evaluated at qsprL. b Probability distribution P x computed from 6=10 disorder realizations for Ls16 at

Ž . Ž a. Ž .


Ž . 4 Ž . Ž .2 3

Fig. 4. a q D q vs. qL along qys0 axis. Data are obtained by averaging over 10 disorder realizations for Ls16, 32, 64, 128, 256

Ž .

at Tds0.2. The solid line is the least square fit. b Fractional variance as a function of the reduced temperature,ts1yKgrK, for Ls32,

3 < <

64, 128, and 256 averaged over 10 disorder realizations. The solid line is a least-square linear fit for t -0.15.


magnetic field . Instead, we use the fluctuation–dis-sipation relation, 2 ²

ˆ ˆ

: ²



: xA lim q h h y h h q yq q yq



q™0 'lim q2C q , 3

Ž .

Ž .

2 q™0


Ž .

where hq is the Fourier transform of h r . x only

probes the system at the largest scale and is indicated

Ž .

by the q™0 limit, which is evaluated at q ,q s

x y

ŽprL,0 for finite systems..

Ž .

As shown in Fig. 3, the distribution P x at low

temperature is peaked at zero and decays more

strongly than any power laws for large x’s. This

indicates that the glass phase is typically rigid against the penetration of additional fluxlines when the ex-ternal magnetic field is increased by a small amount.

The mean value x, which takes on a finite value


due to the statistical rotational symmetry

w9,15 , is however, controlled by the rare eventsx Ž .

contained in the tail of P x . This is similar to the

behavior found for a single flux line in 1q1 dimen-w x

sional random potential 16,17 .

A striking feature of this vortex glass concerns the sample-to-sample variation of the susceptibility x. It

w x

was predicted 9 that the fractional variance, L™`

2 < <



var x rx ™ Dt for 0-yt<1,

Ž .


is universal, with D being a computable,

size-inde-Ž .

pendent constant of order unity. Using Eq. 3 , we

w x 4 4Ž . Ž .

obtain var x Alimq™ 0q C q where C q4


2 Ž . 4 Ž .


Ž .

q yC2

Ž .

q . As shown in Fig. 4 a , q C q4

4 Ž . Ž .0.78Ž2.

obeys a power-law scaling as q C q4 ; qL

for small q. This behavior is consistent with the analytical prediction that the variance is

size-inde-pendent because the q™0 limit is evaluated at

Žq , qx y.sŽprL,0 for finite systems. The power-law.

scaling and its exponent are, however, not under-stood at present. Finally, the temperature dependence

Ž .

of the fractional variance, as shown in Fig. 4 b , can

be deduced from the relation between Ky1

and Td

Ž .

given in Fig. 2 b . It is well described by the linear

Ž .

form 4 close to the glass transition with Ds

Ž .

0.454 5 .

5. Conclusion

Finite temperature simulations were performed on a disordered dimer model to study the magnetic response of a planar vortex array. Universal suscepti-bility variations in the collective pinning regime were observed; critical behavior near the glass transi-tion compared well with analytic predictransi-tions. It is hoped that the present study will stimulate further experimental investigations of the physics of meso-scopic vortex systems.


w x1 G. Blatter et al., Rev. Mod. Phys. 66 1994 1125.Ž .

w x2 E. Akkermans Ed. , Mesoscopic Quantum Physics, North-Ž .


w x3 C.A. Bolle et al., Nature 399 1999 43.Ž .

w4a J.L. Cardy, S. Ostlund, Phys. Rev. B 25 1982 6899.x Ž .

w4b J. Toner, D.P. DiVincenzo, Phys. Rev. B 41 1990 632.x Ž .

w x5 M.P. Fisher, Phys. Rev. Lett. 62 1989 1415.Ž .

w x6 T. Nattermann, I. Lyuksyutov, M. Schwartz, Europhys.

Ž .

Lett. 16 1991 295.

w x7 T. Giamarchi, P. Le Doussal, Phys. Rev. B 52 1995 1242.Ž .

w x8 T. Hwa, D.R. Nelson, V.M. Vinokur, Phys. Rev. B 67

Ž1993 1167..

w x9 T. Hwa, D.S. Fisher, Phys. Rev. Lett. 72 1994 2466.Ž .

w10a G.G. Batrouni, T. Hwa, Phys. Rev. Lett. 72 1994 4133.x Ž .

w10b E. Marinari, R. Monasson, J.J. Ruiz-Lorenzo, J. Phys. A 28x

Ž1995 3975..

w10c D. Cule, Y. Shapir, Phys. Rev. Lett. 74 1995 114.x Ž .

w12a P.W. Kasteleyn, Physica 27 1961 1209.x Ž .

w12b M.E. Fisher, J. Math. Phys. 7 1966 1776.x Ž .

w13a N. Elkies, G. Kuperberg, M. Larsen, J. Propp, J. Algebraicx

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Comb. 1 1992 111 and 219.

w13b J. Propp, Urban renewal,http:x rrwww-math.mit.edur;


w14a R.W. Youngblood, D.J. Axe, B.M. McCoy, Phys. Rev. Bx

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21 1980 5212.

w14b C.L. Henley, J. Stat. Phys. 89 1997 483.x Ž .

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