On a development of the phenomenological renormalization group

# On a development of the phenomenological renormalization group

O. Borisenko
Institute for Theoretical Physics, Kiev, Ukraine
E-mail: oleg@bitp.kiev.ua
Speaker.
V. Chelnokov
Institute for Theoretical Physics, Kiev, Ukrainen
E-mail: chelnokov@bitp.kiev.ua
V. Kushnir
Institute for Theoretical Physics, Kiev, Ukrainen
E-mail: vkushnir@bitp.kiev.ua
###### Abstract

We propose a modification of the Nightingale renormalization group for lattice spin and gauge models by combining it with the cluster decimation approximation. Essential ingredients of our approach are: 1) exact calculation of the partition and correlation function on a finite lattice strip; 2) preservation of the mass gap or the second moment correlation length, computed in the infinite strip length limit, on each decimation step. The method is applied for studying general two and three dimensional Z(N) models. A perfect agreement with exact results (whenever available) is found. An extension of the method to models with a continuous symmetry is briefly discussed.

On a development of the phenomenological renormalization group

V. Kushnir

Institute for Theoretical Physics, Kiev, Ukrainen

E-mail: vkushnir@bitp.kiev.ua

\abstract@cs

31st International Symposium on Lattice Field Theory LATTICE 2013 July 29 - August 3, 2013 Mainz, Germany

## 1 Introduction

The Migdal-Kadanoff (MK) renormalization group (RG) [1, 2] had a great impact on the development of the real-space RG methods. Its conceptual and technical simplicity have probably been the main reason of the numerous applications of the MK RG ranging from two-dimensional () classical spin models to the confinement problem in gauge theories. In some special cases like and hierarchical lattices the MK recursion relations (RR) are precise and lead to an exact solutions. In other important cases the MK RG fails to correctly predict the phase diagram of the model, or gives the string tension which is too large [3]. Nevertheless, for a number of physically interesting systems the MK RG does provide qualitatively correct results which however are not very precise on the quantitative level. This fact has impelled people to look for a modification of the original MK transformations which would result in a better quantitative predictions. Indeed, numerous such modifications have been developed in the past.

In the context relevant for this paper we would like to mention an approach to the RG transformations based on the cluster decimation approximation (CDA) [4]. The CDA utilizes the same restructuring of the lattice as in the conventional MK RG. The main idea is to preserve the free energy after each decimation step. This can be done approximately by computing exact free energies on small clusters with periodic boundary conditions (BC), e.g. and . The equality of these free energies is used to establish RR for the effective coupling constant on the lattice. Then, this exact RR is used to approximate the effective coupling constant on new lattice. On this way one gets a considerable improvement of the results over the standard MK RG.

A different class of the RG is represented by a phenomenological renormalization group (PH RG) proposed by Nightingale [5] (for many applications of the PH RG, see [6, 7]). Originally, this approach utilizes the correlation lengths of the partially finite systems. Their scaling relations are then interpreted as the RG equations. When expressed via eigenvalues of the transfer matrix on lattices with different sizes one obtains equations whose solutions approximate the critical temperature and various critical indices.

In the present contribution we develop an approach based on a combination of the PH RG with the CDA. If is a mass gap of the finite system corresponding to a correlation function in representation and is a rescaling factor then in the vicinity of a critical point one has a scaling relation of the simple form . Basically, our approach can be described as follows.

• The relations are treated as a set of equations for new iterated couplings for the whole range of the bare coupling constants;

• In the spirit of the CDA we consider as a cluster the lattice strip , , where is dimension of the system.

Alternatively, one can employ the second moment correlation length to obtain the phenomenological RG equations. This choice provides a good basis for Monte Carlo simulations on the square clusters. In the following we use both the mass gap and the second moment correlation length.

This paper is organized as follows. In Section 2 we outline a general scheme of RG transformations on the example of the general spin models. Here, we also briefly discuss our approach to computation of partition and correlation functions on the finite lattice strips. In Section 3 we present some results of our study for two-and three-dimensional models. In Section 4 we summarise our results.

## 2 Construction of RG transformations

We work on a -dimensional hypercubic lattice with lattice spacing and a linear extension . , denote the sites of the lattice, denote links and is a unit vector in -th direction. We impose periodic BC. will denote lattice obtained after decimation steps with the extension . Here we treat models only with interactions between nearest neighbours. The partition function (PF) of the general model can be written down as

 Z(Λ0,{tk}) = ∏x∈Λ0⎛⎝1NN−1∑s(x)=0⎞⎠ ∏l∈Λ0 Q[{tk};s(x)−s(x+en)] .\specialhtml:\specialhtml: (2.0)

The most general -symmetric Boltzmann weight is defined as

 Q[{tk};s] = N−1∑k=0 tk exp[2πiN k s] .\specialhtml:\specialhtml: (2.0)

The set of coupling constants can be choosen to satisfy

 t0=1 , 0≤tk≤1 , tk=t−k=tk+N . (2.0)

The two-point correlation function in the representation reads

 Γr(Λ0,{tk};R) = ⟨ exp[2πiN r (s(x)−s(x+R))] ⟩ .\specialhtml:\specialhtml: (2.0)

If all couplings are set to be equal, i.e. , one gets the standard Potts model. The coupling constants of the vector Potts model are given by

 tk = Ck/C0 ,  Ck = N−1∑m=0 exp[βcos2πN m+2πiN m k] = ∞∑s=−∞ INs+k(β) .\specialhtml:\specialhtml: (2.0)

Here, is the modified Bessel function.

Our goal is to present both partition and correlation functions on a decimated lattice in the form

 Z(Λ0,{tk}) = A({tk}) Z(Λ1,{t(1)k}) , Γr(Λ0,{tk};R) = Gr({tk},R) Γr(Λ1,{t(1)k};R/2) (2.0)

with unchanged Boltzmann weight and a new set of couplings . Actually, any real-space RG amounts to a prescription of how to (approximately) compute, e.g. constant and new couplings . We propose here to use the CDA of a certain type. We explain the main idea on the example of the two-dimensional lattice taking the rescaling factor . Extension to higher dimensions and to other values of is straightforward.

Let be a strip of a lattice with a width fixed and periodic BC in both directions. Define the free energy and the correlation function in the thermodynamic limit as

 F(M,{tk}) = logλ0(M,{tk}) = limL→∞ 1L logZ(M×L,{tk}) , (2.0) Γr(M,{tk};R) = limL→∞ Γr(M×L,{tk};R) . (2.0)

Suppose that has the following very general form

 Γr(M,{tk};R) = Dr(M,{tk},R) [Br(M,{tk})]R ,\specialhtml:\specialhtml: (2.0)

where the function describing the exponential decay is parametrized as

 Br(M,{tk}) = λr(M,{tk})λ0(M,{tk})\specialhtml:\specialhtml: (2.0)

and the function has utmost a power-like decay. Functions can be considered, e.g. as the eigenvalues of the corresponding transfer matrices. Our basic idea is to present the correlation function via the correlation function , calculated on the strip of the width with new couplings , in the form

 Γr(M,{tk};R) = Dr(M,{tk},R)Dr(M/2,{t(1)k},R/2) Γr(M/2,{t(1)k};R/2) .\specialhtml:\specialhtml: (2.0)

Comparing (2.0) with the last equation one concludes that (2.0) holds if

 B2r(M,{tk}) = Br(M/2,{t(1)k})\specialhtml:\specialhtml: (2.0)

for all . This system of equations determines new couplings on the lattice strip . We use these exact relations to approximate the partition and the correlation functions on as

 Z(Λ0,{tk}) = ⎡⎣λ0(M,{tk})λ(1/2)0(M/2,{t(1)k})⎤⎦L2/M Z(Λ1,{t(1)k}) , (2.0) Γr(Λ0,{tk};R) = Dr(M,{tk},R)Dr(M/2,{t(1)k},R/2) Γr(Λ1,{t(1)k};R/2) . (2.0)

Equations (2.0)-(2.0) and (2.0)-(2.0) define our RG transformations. Renormalized coupling constants are computed from the equation (2.0) which is, of course, the equation of the PH RG. When formulated in such a manner the PH RG becomes much more flexible tool, for it allows to perform many iterations. This is essential for the system with many coupling constants, be it original bare coupling constants or the constants generated during iterations. The second important gain is that within this approach one can compute not only critical characteristics of the system but also many thermodynamical functions in the whole range of the coupling constants. Also, instead of the mass gap preservation one can take any appropriate quantity whose scaling is known. For example, one could work with the second moment correlation length which is more suitable for the numerical Monte-Carlo computations.

Similarly to any RG of this type, the main technical difficulty arises from the desire to obtain as precise results as possible. It is well known that the precision of the results systematically improves when the lattice strip width becomes larger and larger [5]. However, computation of the mass gap on a large strip requires diagonalization of big transfer matrices and this appears to be an important obstacle in the applications of this method. We have designed an original approach to the diagonalization problem details of which will be presented in [8]. Here we briefly outline two main ingredients of our approach.

1. The partition and correlation functions are computed in a dual formulation. E.g., for models one finds

 Z(Λ0,{tk}) = N−1∑rn=0 ∏x∈Λ0⎛⎝1NN−1∑s(x)=0⎞⎠ ∏l∈Λ0 ts(x)−s(x+en)+ηn ,\specialhtml:\specialhtml: (2.0)

where on a set of dual links which forms a closed path due to periodic boundary conditions, and , otherwise. The transfer matrix is constructed in the dual formulation. The largest eigenvalue of the transfer matrix with gives the dominant contribution to the partition function while the largest eigenvalue of the transfer matrix with gives the dominant contribution to the correlation function in the representation in the first direction.

2. The transfer matrix itself is constructed not on the spin configurations but on coefficients describing evolution of all independent couplings. Such couplings are extracted after first direct summation over all spins from a given column in a strip. This approach automatically takes into account all lattice symmetries and significantly reduces the size of the matrix.

With this technics we have been able, for example, to compute the partition and the correlation functions for all standard Potts models up to in the presence of an external magnetic field, and for general models up to at zero magnetic field (to the best of our knoweledge, the partition function for all standard Potts models has been calculated exactly so far on the finite lattice strips for , [9]).

## 3 Application for Z(n) models

Below we list some of the results obtained by applying above procedure to spin models and to lattice gauge theories. More applications together with technical details will be given in a forthcoming paper [8].

Our first example concerns the general spin model. The phase structure of this model is well known so that we can check both the validity and the precision of our approach. Fixed points are extracted from the solution of the recursion relations and the critical lines can be obtained after just several transformations since the RG iterations converge rather fast. Critical index is derived in a usual way by linearising the RG equations around fixed points. In this case we find 4 fixed points corresponding to: 1) the standard Potts model (), 2) the vector model (), 3) and 4) models defined on lines and . Our results are summarised in Table 1 (results for the line reproduce the ones for ).

In our next example we use the second moment correlation length as a quantity which we preserve during RG steps. In this case we consider a square cluster of size and the RG of the form . Table 2 summarises results of our Monte-Carlo simulations for several Potts models. Subscript refers to exact values.

We have also studied the general gauge models for various . In this case we also used duality transformations and performed RG iterations with the smallest cluster . In Table 3 we present the estimates of the critical points , both in standard Potts gauge models and in vector gauge models and compare them with the results of Monte Carlo numerical simulations.

## 4 Summary and perspectives

In this paper we considered a simple modification of the PH RG by combining it with the CDA. Within these frameworks we have derived exact representations for the partition and correlation functions on the decimated lattice. Recursion relations are derived from the requirement of the preservation of the mass gap (or the second moment correlation length) of the system for each representation of the correlation function on every RG iteration. We then presented results of application of this approach to various two- and three-dimensional models. One sees from the Tables given in Section 3 that RG equations obtained even on small lattice clusters give very reasonable approximations to exact or numerical values. Clearly, the above procedure can be easily extended to models with continuous symmetry like the model, the principal chiral model and the sigma model as well as to gauge theories. The details of the corresponding constructions will be given elsewhere.

## References

• [1] A.A. Migdal, Zh. Eksp. Teor. Fiz. 69 (1975) 1457; (Sov. Phys.-JETP 42 (1975) 743).
• [2] L.P. Kadanoff, Ann. Phys. 100 (1976) 359.
• [3] K.R. Ito, Phys.Rev.Lett. 54 (1985) 2383; Phys.Rev.Lett. 55 (1985) 558.
• [4] Raymond E. Goldstein, James S. Walker, J.Phys. A: Math.Gen. 18 (1985) 1275.
• [5] M.P. Nightingale, Physica 83A (1976) 561.
• [6] M.P. Nightingale, J.Appl.Phys. 53 (1982) 7927.
• [7] M.A. Yurishchev, JETP 91 (2000) 332.
• [8] O. Borisenko, V. Chelnokov, V. Kushnir, in preparation.
• [9] Jesus Salas, Shu-Chiuan Chang, Robert Shrock, J. Stat. Phys. 107 (2002) 1207.
• [10] A. Bazavov, B.A. Berg, S. Dubey, Nucl. Phys. B 802 (2008) 421.
• [11] O. Borisenko, V. Chelnokov, G. Cortese, R. Fiore, M. Gravina, A. Papa, I. Surzhikov, [arXiv:1310.5997 [hep-lat]].
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