It is conjectured that the Haldane phase of the S=1 antiferromagnetic
Heisenberg chain and the $S=1/2$ ferromagnetic-antiferromagnetic alternating
Heisenberg chain is stable against any strength of randomness, because of
imposed breakdown of translational symmetry. This conjecture is confirmed by
the density matrix renormalization group calculation of the string order
parameter and the energy gap distribution.Comment: 4 Pages, 7 figures; Considerable revisions are made in abstract and
  main text. Final accepted versio

B. Boechat

C. Dasgupta

C. Monthus

D. S. Fisher

E. Westerberg

H. Tasaki

K. Hida

Kazuo Hida

L. P. Regnault

M. A. Constantino

M. den Nijs

M. Hase

R. A. Hyman

R. N. Bhatt

S. R. White

S.-k. Ma

Y. Nishiyama

English

arXiv

It is conjectured that the Haldane phase of the S = 1 antiferromagnetic Heisenberg chain and the S = 1/2 ferromagnetic-antiferromagnetic alternating Heisenberg chain is stable against any strength of randomness, because of imposed breakdown of translational symmetry. This conjecture is confirmed by the density matrix renormalization group calculation of the string order parameter and the energy gap distribution

飛田 和男

Saitama University Cyber Repository of Academic Resources

VOLUME 83, NUMBER 16 P H Y S I C A L R E V I E W L E T T E R S 18 OCTOBER 1999Density Matrix Renormalization Group Study of the Haldane Phasein Random One-Dimensional AntiferromagnetsKazuo HidaDepartment of Physics, Faculty of Science, Saitama University, Urawa, Saitama 338-8570, Japan(Received 24 February 1999)It is conjectured that the Haldane phase of the S  1 antiferromagnetic Heisenberg chain and theS  12 ferromagnetic-antiferromagnetic alternating Heisenberg chain is stable against any strength ofrandomness, because of imposed breakdown of translational symmetry. This conjecture is confirmedby the density matrix renormalization group calculation of the string order parameter and the energygap distribution.PACS numbers: 75.10.Jm, 64.60.Ak, 75.40.Mg, 75.50.–yIn the recent studies of the quantum many body problem,the ground state properties of the random quantum spinsystems have been attracting a renewed interest [1–15].Among them, the effect of randomness on the spin gapstate of quantum spin chains has been extensively studiedtheoretically and experimentally [5–15].The real space renormalization group (RSRG) methodhas been often used for the study of random quantumspin chains. Using this method, it has been exactlyproved that the ground state of the S  12 randomantiferromagnetic Heisenberg chain (RAHC) is the ran-dom singlet (RS) state [1–3] irrespective of the strengthof randomness. Hyman et al. [5] have applied thismethod to the S  12 dimerized RAHC and haveshown that the dimerization is relevant to the RS phase.They concluded that the ground state of this modelis the random dimer phase in which the string longrange order survives even in the presence of randomness[5,8]. These results are numerically confirmed using thedensity matrix renormalization group (DMRG) method[4,9].The effect of randomness on the Haldane phase is alsostudied by Boechat and co-workers [6,7] and Hyman andYang [8] using the RSRG method for the original modeland the low energy effective model, respectively. Theseauthors predicted the possibility of the RS phase for strongenough randomness. This problem has been further stud-ied by Monthus and co-workers using the numerical analy-sis of the RSRG equation for the square distribution ofexchange coupling [10]. They predicted that the Haldane-RS phase transition takes place at a finite critical strengthof randomness. In the finite neighborhood of the criticalpoint, the Haldane phase belongs to the Griffith phase withfinite dynamical exponent z . 1. Hereafter, this phaseis called the random Haldane (RH) phase. On the otherhand, Nishiyama [11] has carried out the exact diagonal-ization study of the S  1 RAHC. He observed that theHaldane phase is quite robust against randomness and thestring order remains finite unless the bond strength is dis-tributed down to zero. He also carried out the quantumMonte Carlo simulation [12] and found no random sin-0031-90079983(16)3297(4)$15.00glet phase even for strong randomness. On the contrary,the quantum Monte Carlo simulation by Todo et al. [13]suggested the presence of the RS phase for strong enoughrandomness.In the absence of randomness, the present author hasgiven a physical picture of the Haldane phase as the lim-iting case of the S  12 Heisenberg chain with bondalternation in which the exchange coupling takes two dif-ferent values J and JF alternatingly [16]. In the extremecase of JF ! 2`, this system tends to the S  1 an-tiferromagnetic Heisenberg chain. The string order re-mains long ranged over the whole range 2` , JF , Jand vanishes only at J  JF . The perfect string order isrealized for JF  0. As discussed by Hyman et al. [5],this is the direct consequence of the imposed break-down of translational symmetry. Because the randomnesscannot recover the translational symmetry, the string orderis expected to remain finite over the whole range 2` ,JF , J for any strength of randomness. Therefore wemay safely conjecture that the Haldane phase of the S  1RAHC should also remain stable for any strength ofrandomness.In the following, we confirm this conjecture using theDMRG method [4,17] which allows the calculation of theground state and low energy properties of large systemswith high accuracy. We use the algorithm introduced inRef. [4]. This method has been successfully applied to thespin-12 RAHC and weakly dimerized spin-12 RAHC inwhich the system is gapless or has a very small gap inthe absence of randomness. Namely, in these systems thecharacteristic energy scale of the regular system is muchsmaller than the strength of randomness even for weakrandomness. Compared to these examples, the presentmodel is less dangerous because the regular system hasa finite gap and the characteristic energy scale of theregular system is comparable to the strength of randomnesseven in the worst case. We investigate not only the S 1 RAHC but also the S  12 random ferromagnetic-antiferromagnetic alternating Heisenberg chain (RFAHC)which interpolates the S  12 dimerized RAHC and theS  1 RAHC.© 1999 The American Physical Society 3297VOLUME 83, NUMBER 16 P H Y S I C A L R E V I E W L E T T E R S 18 OCTOBER 1999The Hamiltonian of the S  12 RFAHC is given byH NXi12JiS2i21S2i 1 2JFS2iS2i11, jSij  12 ,(1)where JF  const and Ji’s are distributed randomly withprobability distribution,PJi Ω1W for 1 2 W2 , Ji , 1 1 W20 otherwise. (2)The width W of the distribution represents the strengthof randomness. The maximum randomness is defined byW  2, because the ferromagnetic bonds appear amongJi’s for W . 2. It should be noted that the appearanceof the random ferromagnetic bonds can drive the systemto the completely different fixed point called large spinphase [18]. Although the crossover between the randomHaldane phase and the large spin phase is an interestingissue, we leave this problem outside the scope of thepresent study.The ground state of the regular counterpart of thismodel (W  0) is the Haldane phase with long rangestring order defined by Ostr  liml,N!`Ostrl;N [16].Here, Ostr l;N is the string correlation function in thechain of length N defined only for odd l asOstrl;N  24*exp(ip2i1l11Xk2i11Szk)+. (3)where · · · denotes the ground state average. In thepresence of randomness, the string order is defined as thesample average of Ostr . In the limit JF ! 2`, the stringorder parameter (3) reduces to the one for the S  1 chain[19,20].First, we calculate Ostr for the S  12 RFAHC andS  1 RAHC using the DMRG method. The calculationis performed with an open boundary condition. Forthe S  12 RFAHC, the bonds at both ends of thechain are chosen to be antiferromagnetic to avoid thequasidegeneracy of the ground state. The two boundaryspins are not counted in the number of spins 2N tokeep the consistency with the S  1 chain (see below).The average is taken over 200 samples with N # 29(58 spins). The string order for the finite system Ostr Nis estimated from Ostr l;N averaged over six values ofl around l  N2. The maximum number m of thestates kept in each step is 100. Similar calculation isalso performed for the S  1 RAHC. In this case, theadditional spins with S  12 are added at both ends ofthe chain to remove the quasidegeneracy as proposed byWhite and Huse for the regular chain [21]. The averageis taken over 400 samples with N # 42, where N is thenumber of S  1 spins. In this case, we take m  80,and Ostr N is estimated from Ostrl;N averaged over12 values of l around l  N2. We have confirmedthat these values of m are large enough from the mdependence of the obtained values of Ostr N.3298Figure 1 shows the size dependence of the string order.Typical sizes of the error bars estimated from the statisticalfluctuation among samples are less than the size of thesymbols unless they are explicitly shown in the figures.The extrapolation is made under the following assumption:OstrN  Ostr 1 CN22h exp2Nj , (4)whereC and j are the constants to be determined by fitting.The exponent 2h characterizes the size dependence ofthe string order parameter at the RH-RS critical pointwhere j should diverge as Ostr N  N22h . This valueis estimated as follows: According to Monthus et al. [10],at the critical point, Ostr N behaves as G2232f withf p5 while the logarithmic energy scale G varieswith the system size as G  N13. Therefore Ostr Nshould scale as N2232f3  N20.5092 at the critical pointresulting in 2h  0.5092. It should be noted that thelow energy effective model of Hyman and Yang [8] alsoapplies for the S  12 RFAHC with finite JF , 0 byconstruction. The extrapolated values of Ostr are plottedagainst 1jJF j in Fig. 2. The string order is perfect atJF  0, where the ground state is a simple assembly oflocal singlets [16] and should decrease with the increaseof jJF j. This behavior is clearly seen in Fig. 2. In thisextrapolation scheme, the string long range order remainsfinite even at W  2 for both S  12 RFAHC andS  1 RAHC.To check our extrapolation scheme, we also madethe extrapolation assuming the size dependence N22hexpected at the RH-RS critical point in Fig. 3 for S  1RAHC. In the RH phase, the extrapolated values thusobtained can be understood as the lower bound. ForW $ 1.9, it is clear that the extrapolated values remaindefinitely positive. Therefore the extrapolation usingEq. (4) is appropriate in this region rather than the power0 0.02 0.0400.250.50.75JF=–2–4–8–161/NOstr(N)W=1.61.81.92.0 S=1FIG. 1. The size dependence of the string order parameterOstr N plotted against 1N . The solid lines are fit by theformula (4). The points with different values of W are depictedby the same symbols for W  1.6, 1.8, 1.9, and 2.0 from topto bottom.VOLUME 83, NUMBER 16 P H Y S I C A L R E V I E W L E T T E R S 18 OCTOBER 19990 0.1 0.200.5Ostr1/|JF|1.61.81.92.0W=0 regularFIG. 2. The JF dependence of the string order parameter Ostrfor W  1.6, 1.8, 1.9, and 2.0 plotted against 1jJF j.law extrapolation. For W  2, the extrapolated value isvery small but still positive ( 0.018).Even if we do not rely on the values for W  2extrapolated using Eq. (4), we can convince ourselves ofthe stability of the RH phase at W  2 by the followingargument. In Fig. 4, we plot Ostr extrapolated usingEq. (4) for S  1 RAHC against 2 2 W for W # 1.9.If we assume the critical behavior Ostr  Wc 2 W1.173predicted by Monthus et al. [10], it is highly unlikelythat the string order disappears at finite values of Wc lessthan 2.Especially, this excludes the possibility Wc  1.485predicted by Monthus et al. [10]. In general, it is notsurprising that the RSRG method gives an incorrect valuefor the critical point even if it gives correct values forthe critical exponents, because the RSRG transformationis not exact at the initial stage of renormalization. Fur-thermore, Monthus et al. [10] have neglected the effectiveferromagnetic coupling between the next nearest neigh-bor interaction which appears after decimation of twoS  1 spins. [See the discussion following Eq. (2.20) ofRef. [10].] The neglect of this term is equivalent to theintroduction of the antiferromagnetic next nearest neigh-bor interaction as a counterterm in the bare interaction. Interms of the RFAHC, such interaction makes the distinc-tion between the even and the odd bonds meaningless andFIG. 3. The size dependence of the string order parameterOstr N for the S  1 RAHC plotted against N20.5092.0 0.2 0.400.10.20.32–WOstrFIG. 4. The W dependence of the string order parameter Ostrfor the S  1 RAHC.can recover the translational symmetry leading to the de-struction of the string order erroneously.To further confirm the stability of the RH phase at themost dangerous point JF ! 2` and W & 2, we calculatethe energy gap distribution for the S  1 RAHC. In theRH phase, the fixed point distribution of the energy gap Dis given by Px  P0 exp2P0x, where x  lnVD,V is the energy cutoff, and P0 is the nonuniversal constant[8]. For the finite size systems, V scales as N21P0 [8].Therefore the dynamical exponent z is given by z  1P0.Furthermore, this distribution impliesln1D  P210 lnN 1 const, (5)s qlnD 2 lnD2  P210  z , (6)for N ¿ 1. In Fig. 5, we plot ln1D and s againstlnN . The error bars are estimated from the statistical fluc-tuation among samples. The average is taken over morethan 100 samples with N # 50. For the most random caseW  2, the average is taken over 219 samples. In thiscase, we have taken m  100 in most cases. For the con-firmation of the accuracy, however, we recalculated with2 3 40246lnN<ln(1/∆)>   σW=2  1.9  1.8FIG. 5. The N dependence of ln1D (open symbols) ands (filled symbols) of the S  1 RAHC plotted against lnNfor W  1.8, 1.9, and 2.0. The horizontal arrows indicate thevalues of 1P0 estimated from dln1Dd lnN for W  2,1.9, and 1.8 from top to bottom.3299VOLUME 83, NUMBER 16 P H Y S I C A L R E V I E W L E T T E R S 18 OCTOBER 19992 3246N1/3<ln(1/∆)>W=2  1.9  1.8(a)2 4 6246N1/2<ln(1/∆)>W=2  1.9  1.8(b)FIG. 6. The N dependence of ln1D of the S  1 RAHCplotted (a) N13 and (b) N12 for W  1.8, 1.9, and 2.0.m  150 for the samples with very small gap (less than1023) but the difference was negligible. Actually, the lat-ter data are also plotted in Fig. 5 for W  2. But they arealmost covered by the data with m  100 and are invisiblein Fig. 5. Therefore we may safely neglect the m depen-dence for the less dangerous case W , 2.It is evident that ln1D behaves linearly with lnN ,and s tends to a constant value as N ! `. We canestimate the values of z  1P0 from the gradientdln1Dd lnN for large N . These values are indicatedby the arrows in Fig. 5 and they are consistent with thoseestimated from s for large N within the error bars. Onthe other hand, Figs. 6(a) and 6(b) show the plot ofln1D against N13 and N12 which are the expectedsize dependence at the RH-RS critical point and withinthe RS phase, respectively [10]. Both plots are less linearcompared to Fig. 5. These results confirm that the groundstate of the S  1 RAHC remains in the RH phase downto W  2.It should be also noted that the finite size effectbecomes serious only if one hopes to conclude thepresence of the RS phase. Even in the RH phase, thestring order or the gap distribution might behave RS-likeif the system size is not enough. Actually, the authorsof Ref. [10] needed an extremely large number of spinsto conclude that their calculation leads to the RS phase.But the RS phase can never behave RH-like by the finitesize effect because the RS phase has divergent correlation3300length. Therefore, it is relatively easy to exclude thepossibility of the RS phase if the deviation from theRS-like behavior is already observed for relatively smallsystems, which is the case of the present calculation.In summary, it is conjectured that the Haldane phaseof the S  1 RAHC and the S  12 RFAHC is stableagainst any strength of randomness, because of theimposed breakdown of translational symmetry. Thisconjecture is confirmed by the DMRG calculation of thestring order and the energy gap distribution.The numerical calculations have been performed usingthe FACOM VPP500 at the Supercomputer Center, Insti-tute for Solid State Physics, University of Tokyo. Theauthor thanks H. Takayama and S. Todo for useful dis-cussion and comments. This work is partially supportedby the Grant-in-Aid for Scientific Research from the Min-istry of Education, Science, Sports and Culture.[1] S.-k. Ma, C. Dasgupta, and C. K. Hu, Phys. Rev. Lett. 43,1434 (1979); C. Dasgupta and S.-k. Ma, Phys. Rev. B 22,1305 (1980).[2] R. N. Bhatt and P. A. Lee, Phys. Rev. Lett. 48, 344 (1982).[3] D. S. Fisher, Phys. Rev. B 50, 3799 (1994).[4] K. Hida, J. Phys. Soc. Jpn. 65, 895 (1996); J. Phys. Soc.Jpn. 65, 3412(E) (1996).[5] R. A. Hyman, K. Yang, R. N. Bhatt, and S. M. Girvin,Phys. Rev. Lett. 76, 839 (1996).[6] B. Boechat, A. Saguia, and M. A. Continentino, SolidState Commun. 98, 411 (1996).[7] M. A. Constantino, J. C. Fernandes, R. B. Guimarães,B. Boechat, H. A. Borges, J. V. Vararelli, E. Haanappel,A. Lacerda, and P. R. J. Silva, Philos. Mag. B 73, 601(1996).[8] R. A. Hyman and K. Yang, Phys. Rev. Lett. 78, 1783(1997).[9] K. Hida, J. Phys. Soc. Jpn. 66, 3237 (1997).[10] C. Monthus, O. Golinelli, and Th. Jolicœur, Phys. Rev.Lett. 79, 3254 (1997).[11] Y. Nishiyama, Physica (Amsterdam) 252A, 35 (1998);258A, 499(E) (1998).[12] Y. Nishiyama, Eur. J. Phys. B 6, 335 (1998).[13] S. Todo, K. Kato, and H. Takayama, cond-mat/9803088;(private communication).[14] L. P. Regnault, J. P. Renard, G. Dhalenne, and A.Revcolevschi, Europhys. Lett. 32, 579 (1995).[15] M. Hase, K. Uchinokura, R. J. Birgeneau, K. Hirota, andG. Shirane, J. Phys. Soc. Jpn. 65, 1392 (1996).[16] K. Hida, Phys. Rev. B 45, 2207 (1992).[17] S. R. White, Phys. Rev. Lett. 69, 2863 (1992); Phys. Rev.B 48, 10 345 (1993).[18] E. Westerberg, A. Furusaki, M. Sigrist, and P. A. Lee,Phys. Rev. Lett. 75, 4302 (1995); Phys. Rev. B 55, 12 578(1997).[19] M. den Nijs and K. Rommelse, Phys. Rev. B 40, 4709(1989).[20] H. Tasaki, Phys. Rev. Lett. 66, 798 (1991).[21] S. R. White and D. A. Huse, Phys. Rev. B 48, 3844 (1993).

Density matrix renormalization group study of the haldane phase in random one-dimensional antiferromagnets

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