# Partial annealing of a coupled mean-field spin-glass model with an embedded pattern

###### Abstract

A partially annealed mean-field spin-glass model with a locally embedded pattern is studied. The model consists of two dynamical variables, spins and interactions, that are in contact with thermal baths at temperatures and , respectively. Unlike the quenched system, characteristic correlations among the interactions are induced by the partial annealing. The model exhibits three phases, which are paramagnetic, ferromagnetic and spin-glass phases. In the ferromagnetic phase, the embedded pattern is stably realized. The phase diagram depends significantly on the ratio of two temperatures . In particular, a reentrant transition from the embedded ferromagnetic to the spin-glass phases with decreasing is found only below at a certain value of . This indicates that above the critical value the embedded pattern is supported by local field from a non-embedded region. Some equilibrium properties of the interactions in the partial annealing are also discussed in terms of frustration.

###### pacs:

89.20.-a, 75.50.Lk^{†}

^{†}preprint: APS/123-QED

## I Introduction

Spin-glass (SG) models Mzard et al. (1987); Nishimori (2001) have been extensively applied to widespread fields for describing random or randomized spin systems. In such a system, there are two dynamical variables, fast and slow variables that are spins and interactions in a spin model, respectively. The latter is usually assumed to be quenched for simplicity, and is distributed independently and identically according to a given distribution. This is based on the fact that the relaxation time of the interactions is considerably larger than that of the spins. As a result of the quenched randomness, the state of the interactions is not affected at all by the fluctuation of spins. The randomness of the interactions causes many competitions between the spins, and sometimes there is no way for eliminating them completely. This competition that is called frustration provides rich and interesting phenomena in the random systems.

The quenched randomness is an appropriate assumption for a spin-glass problem as a magnetic material. In some interesting systems, however, the fluctuation of the spin variables has large influence on the interaction variables. For example, the interactions of amino-acid sequences provide a globally stable state in the protein. The existence of such global attraction in the folding process was proposed as a consistency principle Go (1983) or funnel landscape Onuchic and Wolynes (2004). The characteristics of interactions are not expected in randomly constructed interactions. It is supposed that such characteristics are acquired through an evolutional process under some fluctuations of the fast variables. In the case of the protein, the fluctuation is due to the folding dynamics of the amino-acid sequences. Similar properties have also been discovered in gene regulatory networks Li et al. (2004) and transcriptional networks Alon (2000). The formation mechanism of the funnel landscape is still not fully understood.

Recently, an adiabatic two-temperature spin model has been studied as a model of evolution by using Monte Carlo simulations Sakata et al. (2009, 2009). In the model, interactions evolved so as to increase the probability of spins to find a specific pattern of local spins. Interestingly, adapted interactions that exhibit funnel-like dynamics with some robustness have been found only in an intermediate temperature region. This type of interactions has no frustration around the local spins and retains some frustrations in the rest. The fact implies that the local spin pattern is stabilized in the adapted interactions by energetic and entropic effects. Note that there is no explicit driving force for constructing interactions outside the local spins. Unfortunately, since numerical simulations are often hampered by finite-size effects, thermodynamic properties and phase structure have not yet been understood well. We consider it worthwhile to clarify the nature of such self-organized interactions with an local spin pattern under the thermal fluctuations from the viewpoint of a statistical-mechanics.

In contrast to the quenched system, a feedback from the fast variables to the slow ones is taken into account for studying such systems. The feedback effect is essential for the emergence of some functional feature in the evolutional process. Under the assumption of the complete separation of time-scales between the fast and slow variables, the adiabatic elimination of fast variables has been employed in non-equilibrium and non-linear physics Nordholm and Zwanzig (1974); Kaneko (1981). One of such approaches, called partial annealing Dotsenko et al. (1994), is introduced by Penney et. al. Penney et al. (1993), in which the fast and slow variables touch with different heat baths and a non-equilibrium system is mapped onto a particular equilibrium statistical-mechanical system with two temperatures. The partial annealing approach has been applied to many topics; a model of glasses Allahverdyan et al. (2000), charged system Mamasakhlisov et. al. (2008), spin-lattice gas CHNakajima (2008), neural network Uezu et.al. (2009), protein-folding Rabello et al. (2008), liquid crystal LiquidCrystal (2010) and evolution Ciliberti-Martin-Wagner (2007); Ancel and Fontana (2000).

In this paper, we study a coupled mean-field spin-glass model Takayama (1992) in the partial annealing. In this model, two fully-connected mean-field systems are coupled with each other through spin-glass interactions. One of them is a ferromagnetic system regarded as a local region in which a ferromagnetic pattern is embedded. The other is a spin-glass system providing redundant interactions together with the coupled interactions. We formulate the mean-field theory for this model in partial annealing and discuss how the redundant interactions are modified by the thermal fluctuation of spins.

This paper is organized as follows. In section II, we introduce a mean-field spin-glass model studied in detail and give a theoretical formulation of the model in the partial annealing by using the replica method. In section III, we present phase diagram of the model and discuss the equilibrium state of interactions through frustration. Finally, section IV is devoted to conclusions and outlook for further developments.

## Ii Model and replica method

We study a coupled mean-field spin-glass model of two fully connected spin systems, which consists of Ising spins and Ising spins . The spin variables of the two systems and the interactions between two spins are denoted by and for short, respectively. The Hamiltonian of the model is given by

(1) |

where the summation in the first term is over all pairs within each spin system and the summation in the second term is over all and . and , denoted hereafter by and , respectively, are the intra-interactions within each system and denoted by are inter-interactions between these two systems. A schematic picture of the model is shown in Fig. 1. In a quenched system, they are assumed to be independently and identically distributed according to the Gaussian distribution with mean and variance ,

(2) |

where the order of interactions is scaled as for keeping the Hamiltonian extensive and is set to be the geometrical mean of and as Takayama (1992).

In this paper, we consider that an ordering pattern is embedded in one of the system (system 1) and no a prior pattern is introduced in the other system (system 2). This is represented by a specific case of the model Hamiltonian, in which the system 1 and the system 2 are a pure ferromagnetic and spin-glass systems, respectively, and they are coupled with each other through spin-glass interactions. Explicitly, the model is given as

(3) |

Note that in the model with these parameters the interactions and are expected to be modified by the partial annealing while is kept to be fixed to the pure ferromagnetic interaction. A size ratio between the two systems is defined as

(4) |

yielding that and with the total number of spins . Two limiting cases and correspond to the Husimi-Temperley model and the Sherrington-Kirkpatrick model, respectively.

In the partial annealing system, the interactions as well as the spin variables are treated as a dynamical variable. Time scales associated with is extremely slow and it is assumed that the time scale is separated from that of the spin variables. Then, the equilibrium distribution of the spins at an inverse temperature is given by

(5) |

where is a partition function under a given . The distribution function of at an inverse temperature , different from , is given by

(6) |

where is a Hamiltonian of and is the total partition function. The Hamiltonian of is generally expressed in terms of equilibrium quantities of and the bare distribution of Eq. (2). Although the explicit form of can be arbitrary chosen, in this study, as in Penney et al. (1993); Dotsenko et al. (1994), we set it as

(7) |

where is the free energy defined by and .

Then, the equilibrium distribution and the total partition function are rewritten as

(8) | |||||

(9) |

where is the ratio between two temperatures, , and means the average over according to the bare distribution . When , the distribution is identical to and the system corresponds to the quenched one. For finite and , the interactions with a lower free energy likely occur.

In the quench limit, the model is reduced to that studied by Takayama Takayama (1988, 1992). The coupled mean-field model has been introduced in order to study inhomogeneity of interactions between spins in real SG materials Takayama (1988, 1992). Thus, the previous studies focused attention only on the quenched system. In this work, we rather pay attention to the system with the partial annealing, in which the interactions except for the embedded one in system 1 are adiabatically affected by fluctuations of spins. Our main purpose is to study the partial annealing effect on the stability of the embedded ferromagnetic ordering in the system 1 and to clarify characteristics of the resultant interactions by the partial annealing.

The total free energy per spin at two inverse temperatures and can be written as

(10) |

Following the standard procedure of the replica method Mzard et al. (1987), the quantity is calculated for a positive integer and an analytic continuation to a real value given by two temperatures is taken after the calculation. Within the assumption of replica symmetry, the free-energy density is described in terms of order parameters , and , and their conjugate parameters , and , as

(11) |

where , and . The order parameters follow the self-consistent equations,

(12) |

and

(13) |

where and . The conjugate parameters, , and , are then given by

(14) |

By solving the self-consistent equations we have the following solutions: paramagnetic solution , ferromagnetic one , and spin-glass one . The transition temperatures between two of the phases corresponding to these solutions are given by

(15) | ||||

(16) | ||||

(17) |

where PM, FM and SG mean paramagnetic, ferromagnetic, and spin-glass phase, respectively. The phase boundary between the paramagnetic phase and the spin-glass one and that between the paramagnetic phase and the ferromagnetic one are independent of and . Thus, the multicritical point located on in the plane is independent of and . They are consistent with the previous work in the quench limit Takayama (1992).

By following the stability analysis of the RS solutions by de Almeida and Thouless (AT) Almeida (2000), the stability condition is derived as

(18) |

where

(19) |

## Iii Results

### iii.1 Phase diagram

As shown in the previous subsection, the transition temperature between the ferromagnetic and spin-glass phases depends on the characteristic parameters and of our model. Here we carefully discuss and -dependence of the phase boundaries. To completely obtain the phase boundary of , we should numerically solve the self-consistent equations Eq. (12) and Eq. (13). Some limit cases around multicritical point and near can be argued by an expansion of the order parameters.

At sufficiently low , the spin-glass order parameters for and 2 behave as

(20) |

where and . They decrease from 1 exponentially in for and linearly in for . Substituting them into Eq. (15), we find that around , irrespective of , and that the RS solution at always satisfies the stability condition (18). Therefore, at the ferromagnetic phase stably exists for any and and it vanishes at . The latter is recovered to the quench limit studied in Takayama (1992). At sufficiently low , the partial annealing effect yields the ferromagnetic ordering even for weak and for small ratio by appropriately selecting and . The stability of the ferromagnetic phase near is a particular feature of the partial annealing system of the coupled mean-field model.

Near the multicritical point, the spin-glass order parameters can be expressed as

(21) | ||||

(22) |

The critical exponent of the spin-glass order parameter is 1 at and at . For , the order parameter is difficult to obtain by an expansion because the transition is of first order. The phase boundary around the multicritical point significantly depends on , in contrast to that around .

The phase diagrams at for and are shown in Fig. 2 as an example for . The obtained phase diagram weakly depends on ; for , as decreases the transition from the paramagnetic to ferromagnetic phases occurs at , and for , the spin-glass phase appears at . All the phases found for fulfill the stability condition (18). In particular, the obtained spin-glass phase is correctly described by the RS solution. It would be interesting to see that the region of the spin-glass phase for is reduced as compared with that for . More concretely, the transition temperature around the multicritical point for is lower than that for . This is a counter-intuitive result because in the case with the majority spins in the system 2 connect with each other through the spin-glass interactions while the majority spins are ferromagnetically coupled in the system 1 in the case with . We shall discuss this point later.

In addition to the phases found for , other phases appear for , that are the mixed phase characterized by the AT instability with and spin-glass phase with replica symmetry broken(RSB). The phase diagram at as a typical example for is shown for and in Fig. 3. The mixed phase is found between the ferromagnetic and spin-glass phases and the region of the mixed phase is enlarged with increasing . The region of the spin-glass phase is also enlarged with and a broken replica symmetric phase exists in the intermediate region in the spin-glass phase, in contrast to that observed for . For , a reentrant transition (PMFMMixed) occurs at . Furthermore, the transition from the spin-glass or mixed phases to ferromagnetic phase occurs at lower , because the ferromagnetic phase is always stable at in our model for any finite . Hence, we can see three successive transitions, PMFMMixedFM for .

### iii.2 Reentrant transition

While a characteristic feature of our model is found near , another feature is there around the multi-critical point in the phase diagram. As seen in Fig. 3(b), a reentrant transition from the ferromagnetic to a mixed and spin-glass phases occurs near the multicritical point for . This means that the embedded ferromagnetic ordering of the system 1 described by the RS solution becomes unstable as decreases. Such a reentrant transition has been already reported for the quenched system with Takayama (1992). In this work, we study a partial annealing effect, namely with finite , on the stability of the embedded ferromagnetic ordering. The gradient of at the multicritical point is regarded as an indicator of the “reentrant transition”. Namely, the negative slope of at the multicritical point implies the existence of the reentrant transition, although the existence of a reentrant transition at temperature lower than the multicritical point is not completely ruled out even in the case with positive slope of .

The reentrant transition can occur when the condition

(23) |

is satisfied where and “MCP” means the multicritical point. Note that the order parameter is a function of . The RS solution for is sufficient for evaluating the boundary, because the RS solution is always stable at the multicritical point. From Eq. (23), the region of where the reentrant transition occurs is derived as

(24) |

where the critical ratio is given by

(25) |

For , the reentrant transition occurs at with being a negative value, hence it is unphysical. The derivation of is based on the assumption that the transition is of the second order. Certainly the transition is of second order for , which is larger than . Therefore, the reentrant transition occurs only for . We show -dependence of in Fig. 4. At the smaller , the reentrant transition occurs at smaller . Eventually, takes in the quench limit , that is consistent with the results in Ref. [Takayama, 1992]. Furthermore, it is found that the gradient at the multicritical point is a monotonically increasing function of for , and this fact yields the shrink of the spin-glass phase as increases, as shown in Fig. 2. Thus, the stability of the embedded ferromagnetic ordering of the system 1 depends quantitatively on the value of that is a relative temperature .

Here, we argue a typical feature of the partially annealed interaction from the obtained phase diagram and the critical ratio . In equilibrium of the partial annealing system, the interactions are in general proportional to given as a most probable value in . Supposing that the order parameter of the system 2 has a finite value at sufficiently low temperature , the spins in the system 1 are subjected to an effective field caused by the system 2 through the interactions . For , the interactions are considered to be almost random according to the bare distribution , and hence an effective field is a random field for the system 1. This random effective field also does not favor the ferromagnetic order of the system 1, and the spin glass phase is enhanced as increases. As a consequence of the competition between and , the reentrant transition at is found at . For , the interactions likely have the same sign as . Then, the effective field from the system 2 to the system 1 is not random but it supports the ferromagnetic order in the system 1. Therefore, the ferromagnetic ordering is stabilized even as increases and the system 2 with the spin-glass couplings dominates. The reentrant transition does not occur for any for .

### iii.3 local structures of frustration

In this subsection, we discuss equilibrium properties of the coupled mean-field model from the view point of interactions . Frustration is a key quantity that characterizes a structure of the interactions in spin glasses and related random spin models. It is defined as a product of s along a minimal loop, whose length is three in the fully-connected model studied in this work. If the interactions among three spins satisfy the condition , three terms of the local energy cannot be minimized simultaneously. Such interactions are called to have frustration Toulouse (1977). Meanwhile, all the interactions satisfying do not have frustration and the energy of the spins attains the global minimum value although relative directions of spins are not align totally. This type of interactions is called Mattis model Mattis (1976) and all of the interaction sets can be reduced to the pure ferromagnetic model by local gauge transformation Nishimori (2001).

In the coupled mean-field model, we should consider three distinct frustration parameters originated from three types of interactions, as shown in Fig. 1, are defined;

(26) | ||||

(27) | ||||

(28) |

In equilibrium, these parameters are to be taken average over the equilibrium distribution in Eq. (6) as , and with being the average with respect to . For the limit with kept finite, the distribution is identical to the bare distribution and the average is reduced to . In this limit, the frustration parameters become zero. If the frustration parameters take a positive finite value at finite , this indicates that the frustration is decreased as a consequence of correlation of .

When the bare distribution of the interactions is Gaussian, the averaged frustration parameters are expressed in terms of the order parametersDotsenko et al. (1994); Sakata et al. (2009). In this model, the averaged frustration parameters under the RS ansatz are described as follows,

(29) | ||||

(30) | ||||

(31) |

where and are the eigenvalues of the matrix whose diagonal components are 1 and off-diagonal components are . We can also derive the frustration parameter with multiple step RSB, that does not yield a significant quantitative change Sakata et al. (2009).

At finite , and take a finite value depending on , while zero in the paramagnetic phase. This moderate decrease of the frustration is considered to be due to an emergence of “short-range” correlation of induced by the partial annealing. A considerably qualitative change of the frustration parameters is accompanied by phase transitions. In the spin-glass phase with , and , the frustration parameters and largely increase, but is still zero. Therefore, the frustration is non-uniformly distributed in the system and a “local” structure of frustration is formed; the frustrations in the system 2 and a part of decrease, but a remaining part of has frustration as much as the randomly constituted interactions. The local structure prefers to decrease selectively the frustration of the system 2 in the spin-glass phase, and does not cooperative with the ferromagnetic state of the system 1. Meanwhile, all of the frustration parameters take a positive value in the ferromagnetic phase, because in this phase all order parameters are finite. In this case, all interactions and decrease the energy of the ferromagnetic state of the system 1, meaning that the effective field from the system 2 energetically supports the ferromagnetic state of the system 1. This type of interactions is similar to that of the Mattis states Mattis (1976). These observations of the frustration parameters certify the validity of the argument of and in the previous section.

Before closing this section, we discuss the order of the frustration parameters. The interactions are of order of in the bare distribution. When the frustrations completely vanish with keeping the order of , the order of the frustration parameters become by definition. However, the averaged frustration parameters should be quantities for any , as seen from the expressions Eq. (29), Eq. (30) and Eq. (31). This means that the order of s is appropriately modified to through the partial annealing, and the extensivity of thermodynamic quantities such as energy and free energy is maintained at whole temperature region. It is a characteristic of the partial annealing with the bare distribution function of being Gaussian. When the bare distribution is bimodal and the allowed value of is restricted to , namely model, the order of cannot be changed and the energy becomes in the resultant ferromagnetic phase, that is the lack of extensivity. We should be careful for the study of thermodynamics in such models.

## Iv Summary and discussion

We have studied equilibrium properties of the coupled mean-field model in the partial annealing system, in which the system 1 with an embedded ferromagnetic ordering and the system 2 with no embedded pattern are coupled with spin-glass interactions. In this model, the interactions as well as spins are regarded as dynamical variables, but their time-scales are completely separated from each other. The spins and interactions touch to their own heat bath with different temperatures and . By using the replica method, the free energy of the system is derived as functions of the two temperatures, and the phase diagram is obtained in the two-temperature plane. The phase boundary between the ferromagnetic phase and the spin-glass phase interestingly depends on the model parameters, the size ratio of the system 2 to the system 1 and the ratio between two temperatures.

We carefully studied around the multicritical point. It is found that there exists a critical value in the ratio , which characterizes if the reentrant transition occurs around the multicritical point. For , the partial annealing effect on the inter-coupling is not significant to enhance the embedded ferromagnetic ordering in the system 1. The effective field from the system 2 to the system 1 does not support the ferromagnetic ordering in the system 1. Therefore for a fixed as the ratio increases, in other words the number of spins in the system 2 increases relatively, a competition about the ferromagnetic order is expected; the random filed destabilizes the ferromagnetic order and the coupling stabilizes it. As a result of the competition, the ferromagnetic order is destabilized eventually. This can be seen as the reentrant transition in the phase diagram. Meanwhile, for the effective field supports to achieve the ferromagnetic ordering in the system 1 irrespective of the value of , and the spin-glass region is narrowed monotonically as increases.

We introduced three frustration parameters, , and for characterizing partially annealed interactions of the coupled mean-field model. They are expressed in terms of the order parameters of the spin system in equilibrium. Using the parameters, we classify the type of the interactions in this model into three categories, that correspond to each phase; interactions with a local structure of frustration in the spin-glass phase, Mattis-like interactions in the ferromagnetic phase, and randomly constructed interactions in the paramagnetic phase. The characteristic interactions found in the spin-glass phase do not cooperatively support the ferromagnetic ordering of the system 1, that is to say, the frustration is eliminated from the system 2 independently of the ferromagnetic interactions in the system 1.

This is quite different from those obtained in a related model previously studied Sakata et al. (2009, 2009), in which a locally embedded pattern is supported by the interactions surrounding the pattern and the frustration in the rest of the interactions still remains extensively. Although both models have the same structure that an ordering pattern is embedded in a part of the system, the partial annealing leads to the different property of interactions; the interactions in the previously studied model support the embedded pattern, and those in this study disturb it. A reason of the difference may be originated from the different choice of . In the present work, contains the spin free energy, while in Sakata et al. (2009, 2009) has a local order parameter. The results suggest that an explicit form of strongly affects on the construction of the interaction and the ordering of the spin , in particular, an entropic effect of is nontrivial. For proper understanding of the constructed interactions in the partial annealing, we have to pursue some variant models with a general type of . However, analytical studies of the partial annealing to this time heavily relies on the replica method, that is applicable to only systems with the spin free energy as . The partially annealed system with that does not contain the spin free energy has yet to be revealed in terms of spin-glass theory. An extended formalism of the partially annealed system is required for further applications to biological or engineering models.

In this work, we focus our attention to the mean-field analysis based on the fully connected spin models. When we introduce a diluted model such as the Viana-Bray model VianaBray (1985) in partial annealing, the geometric structure of the partially annealed may play an important role in cooperative phenomenon. Furthermore, a decoupling transition of two degrees of freedom might occur in the diluted models, while the transition of frustration is completely correlated to the transition of the spin variables in our model. Some work in this direction is in progress.

We end with an account of a perspective of the partially annealed system. In most of the studies concerned with the partial annealing, the free energy is used for Hamiltonian of the slow variables . This yields a replicated system with a finite replica number determined by the ratio of two temperatures in the partially annealed system. The partial annealing can be considered to give a physical meaning to the replica approach before taking a limit of the replica number to zero Penney et al. (1993). Meanwhile, the large deviations of the free energy of mean-field spin glasses are studied by the replica method with a finite replica number Parisi and Rizzo (2008). A mechanism of replica symmetry breaking is studied through a phase transition as the replica number is taken to zero TNakajima (2009). Thus, the study of finitely-replicated system can provide new insights into the spin-glass theory. In this work, we discussed a phase transition as a cooperative phenomena of the fast and slow variables with the replica number varying, that might give a different viewpoint to the finitely replicated system. It would be interesting to classify possible universality classes of phase transitions of the finitely replicated systems, particularly in finite dimensions.

###### Acknowledgements.

We would like to thank C. H. Nakajima and T. Nakajima for helpful comments and discussions. This work was supported by a Grant-in-Aid for Scientific Research (No.18079004) from MEXT and JSPS Fellows (No.2010778) from JSPS.## References

- Mzard et al. (1987) M. Mzard, G. Parisi, and M. A. Virasoro, Spin Glass Theory and Beyond (World Sci. Pub., 1987).
- Nishimori (2001) H. Nishimori, Statistical Physics of Spin Glasses and Information Processing: An Introduction (Oxford Univ. Pr., 2001).
- Go (1983) N. Go, Ann. Rev. Biophys. Bioeng. 12, 183 (1983).
- Onuchic and Wolynes (2004) J. N. Onuchic and P. G. Wolynes, Curr. Opin. Struc. Biol. 14, 70 (2004).
- Li et al. (2004) F. Li, T. Long, Y. Lu, Q. Ouyang, and C. Tang, Proc. Natl. Acad. Sci. USA 101, 4781 (2004).
- Alon (2000) R. Milo, S. Shen-Orr, S. Itzkovitz, N. Kashtan, D. Chklovskii, and U. Alon, Science 298, 824 (2002).
- Sakata et al. (2009) A. Sakata, K. Hukushima, and K. Kaneko, Phys. Rev. Lett. 102, 148101 (2009).
- Sakata et al. (2009) A. Sakata, K. Hukushima, and K. Kaneko, Phys. Rev. E 80, 051919 (2009).
- Nordholm and Zwanzig (1974) K. S. J. Nordholm, and R. Zwanzig, J. Stat. Phys. 11, 143 (1974).
- Kaneko (1981) K. Kaneko, Prog. Theor. Phys. 66, 129 (1981).
- Dotsenko et al. (1994) V. Dotsenko, S. Frantz, and M. Mzard, J. Phys. A: Math. Gen. 27, 2351 (1994).
- Penney et al. (1993) R. W. Penney, A. C. C. Coolen, and D. Sherrington, J. Phys. A: Math. Gen. 26, 3681 (1993).
- Allahverdyan et al. (2000) A. E. Allahverdyan, T. M. Nieuwenhuizen, and D. B. Saakian, Euro. phys. J. B 16, 317 (2000).
- Mamasakhlisov et. al. (2008) Y. S. Mamasakhlisov, A. Ali, and R. Podgornik, J. Stat. Phys. 133, 659 (2008).
- CHNakajima (2008) C. H. Nakajima, and K. Hukushima, Phys. Rev. E 78, 041132 (2008).
- Uezu et.al. (2009) T. Uezu, K. Abe, S. Miyoshi, and M. Okada, J. Phys. A: Math. Theor. 43, 025004 (2010).
- Rabello et al. (2008) S. Rabello, A. C. C. Coolen, C. J. Perez-Vicente and F. Fraternali, J. Phys. A: Math. Theor. 41, 285004 (2008).
- LiquidCrystal (2010) E. do Carmo, D. B. Liarte, and S. R. Salinas, Phys. Rev. E 81, 062701 (2010).
- Ciliberti-Martin-Wagner (2007) S. Ciliberti, O. C. Martin, and A. Wagner, PLoS Comput. Biol. 3, e15 (2007).
- Ancel and Fontana (2000) L. W. Ancel and W. Fontana, J. Exp. Zool. (Mol. Dev. Evol.) 288, 242 (2000).
- Takayama (1992) H. Takayama, J. Phys. Soc. Jpn 61, 2512 (1992).
- Takayama (1988) H. Takayama, Prog. Theor. Phys. 80, 827 (1988).
- Almeida (2000) J. R. L. de Almeida, and D. J. Thouless, J. Phys. A: Math. Gen. 11, 983 (1978).
- Toulouse (1977) G. Toulouse, Commun. Phys. 2, 115 (1977).
- Mattis (1976) D. C. Mattis, Phys. Rev. 56, 421 (1976).
- Sakata et al. (2009) A. Sakata, K. Hukushima, and K. Kaneko, J. Phys.: Conf. Ser. 197, 012003 (2010).
- VianaBray (1985) L. Viana, and A. J. Bray, J. Phys. C 18, 3037 (1985).
- Parisi and Rizzo (2008) G. Parisi, and T. Rizzo, Phys. Rev. Lett. 101, 117205 (2008).
- TNakajima (2009) T. Nakajima, and K. Hukushima, Phys. Rev. E 80, 011103 (2009).