Critical dynamics in systems controlled by fractional kinetic equations

# Critical dynamics in systems controlled by fractional kinetic equations

L. A. Batalov A. A. Batalova Department of Statistical Physics, State University, Ulyanovskaya, 1, 198504, St.Petersburg , Petrodvorets, Russia Department of Atmospheric Physics, Saint-Petersburg State University, Ulyanovskaya, 1, 198504, St.Petersburg , Petrodvorets, Russia
###### Abstract

The article is devoted to the dynamics of systems with an anomalous scaling near a critical point. The fractional stochastic equation of a Lanvevin type with the nonlinearity is considered. By analogy with the model A the field theoretic model is built, and its propagators are calculated. The nonlocality of the new action functional in the coordinate representation is caused by the involving of the fractional spatial derivative. It is proved that the new model is multiplicatively renormalizable, the Gell-Man-Low function in the one-loop approximation is evaluted. The existence of the scaling behavior in the framework of the -expansion for a superdiffusion is established.

###### keywords:
fractional processes, renormalization group, stochastic evolution equations, critical scaling, nonlocal lagrangian
journal: Physica A: Statistical Mechanics and its Applications

## 1 Introduction

The models based on the stochastic processes with continuous time are widely used in modern theories of phase transitions, an atmospheric turbulence and electromagnetism 1 (),2 (),eps_frac_der (). From the thermodynamic point of view these models are characterized by the existence of the temperature such that observed experimental results for and differ significantly termo ().

The object of our investigation are systems governed by stochastic equations in the vicinity of the temperature called the critical point. Problems of an equilibrium statistical physics and a thermodynamics without an explicit time-dependence are called static. Obviously in such systems there are processes the description of energy-dissipation. The description of a critical behaviour in the dynamic models is based on the analogous static case, but it is more complex technically A_model (). In critical dynamics only the models of a Langevin type are considered, i.e. the models with the first time derivative on a field.

Among these models the Ginzburg-Landau dynamic model (the model A in the Galperin and Hoenberg classification scheme sheme ()) proposed by Landau and Khalatnikov for description of a superfluidity is the most interesting . The critical dynamics of the model A was investigated using a dimensional regularization and RG-methods based on the -expansion main_book_c (). The RG method allows to prove the existence of the critical scaling (it is a power-law dependence near a critical point of dynamic correlators) and to obtain corrections for the main exponent Vasiliev ().

For the isotropic system which consists of particles moving under the influence of the random Gaussian distributed forces the base of theoretical analysis is the diffusion equation.

For a classical diffusion in the - dimensional space a particle travels for the time period the distance , where is the Onsager kinetic coefficient, which here can be understood as the diffusion coefficient. This dependence is called a normal scaling. However, the power-law dependence of the displacement with the critical exponent more or less than 1/2 (an anomalous scaling) is observed in some physical systems frac_L ().

For such FDE the corresponding scaling exponent is equal , and fractional derivatives are the generalization of integer derivatives. It allows to apply for a solution of linear equations standard methods the Laplace and Fourier transforms.

In the particular case we obtain the standard equations of the Brownian motion. An exact solution of the linear fractional diffusion equation was found for many processes. Some of them generalise the solutions of the standard diffusion equation with the exponential functions replaced by the Mittag-Leffler function diffusion (). Moreover the class of exact solutions of non-linear diffusion equations and the Fokker-Plank equations expanded very much last time Ant_new (); fokker ().

The RG methods and the ideas about description anomalous scaling with fractional differential equations (FDE) with derivative orders (a time derivative) and (a spatial derivative) were developed in the same time.

In our opinion the application of the renormalization group to the solution fractional differential equations will produce good results.This suggestion bases on the observation, which shows us, that much of the systems demonstrated the critical behaviour have the scaling functions with anomalous exponents. Governing equations of these systems are fractional (for example a developed turbulence ren_frac ()). In our paper the technique of the RG method generalisation on dynamic models with fractional spatial and time derivatives is proposed.

We have developed a technique of a renormalization for an arbitrary stochastic problem with the nonlinearity. The one-loop diagram for the most essential model of the critical dynamics - the model was calculated. We showed, that an analogy with statics took place only for and the independence on and .

This technique is convenient in applications, it is used in the calculation of higher orders, because it is based on the well-developed quantum-field renormalization-group theory Ant_vas (). However, it will be showed in the paper, that for the general analysis and determination of critical regimes the 1-loop approximation is enough. Before now the RG method was applied to a nonequilibrium system usually with an anomalous diffusion in the Wilson recursive equations form A_model (),france (). We emphasize, that in our work it was used the quantum-field renormalization. The critical scaling will be proved, the main exponential function and their dependence on and will be found.

The article construct as follows: in section 2 the stochastic task of the critical dynamics is manifested, and its formulation is given in the field theoretic terms. The section 3 is devoted to the calculation of propagators of this model. In section 4 the model is analysed thoroughly and a transition to the renormalized functional of action in the logarithmic dimension of space is carried out. Below we derived the RG-equations and calculated the Gell-Mann-Low function in the one-loop approximation.

## 2 Formulation of problem

We consider a nonequilibrium system described of the scalar function , where is time, - - dimensional radius vector. All calculations demonstrated in this section are easy generalized on the case, where field is multi-components.

The critical dynamic of field is described by the stochastic Langevin equation:

 ∂tφ=λV(φ)+F (1)

where - variational derivative of the static action functional of time-independence free field , - Onsager transport coefficient, - random external force. For this a Gaussian distribution with zero - mean and covariance

 ⟨F(x,t)F(x′,t′)⟩=2λδ(x−x′)δ(t−t′) (2)

is assumed.

The equality of the double Onsager coefficient and the correlator power provides an agreement with the static case described by the functional . It is consequence of the Fokker-Planck equation for the field distribution function main_book_c ().

The functional potential includes a linear differential operator of the second order (Laplacian) for different generalizations of the Ginzburg-Landau functional (further - the model). Therefore the linear part of the stochastic equation (1) is a linear combination of the first derivative time operator and the second derivative space operator sheme ().

The normal scaling is concluded from Eq. (1) in the leading order and : , where , called the Hurst exponent, which is equal .

We can use Eq.  (1) included instead of the partial time and spatial derivatives the fractional derivatives of orders and related to the Hurst exponent for description of the anomalous diffusion processes with same parameter . For representation of subdiffusion processes the partial time derivative could be changed by the fractional derivative of order (), and in the case of superdiffusion laplacian could be changed by the differential operator of order . In models of turbulent transport the Hurst exponent is greater than and is close to .

Therefore we will find so generalization of the problem (1), that allows to use the fractional derivatives. It is convenient to use the time derivative of order in the Caputo representation with the lower terminal , which is usually chosen from the condition of zero antiderivative main_book_f ():

where is the nearest integer bigger than . This representation provides the Laplace transform as following:

As a generalization of the Laplacian, it is convenient to define the operator in momentum representation, in other words, we will work with its Fourier image. The word ”momentum” here can be understood as a wave vector.

If - order of the spatial derivative and - the so-called fractional Laplacian acting on the function of the Schwartz class laplace () , so that , then

 ^h(k)=kσ^f(k),  k≡|k| (5)

If we can also use the integral representation laplace ():

 (−Δ)σ/2f(x)=C(n,σ)P.V.∫Rdf(x)−f(y)∥x−y∥d+σdy (6)

where P.V. stands for principal value and is a normalization constant. Space has standard euclidean norm .

This allows to apply to diffusion equation Laplace or Fourier transforms. The diffusion equation arising in this way is exactly solvable model diff_new ().

 c0Dαtφ(x,t)=−λ(−Δ)σ/2φ(x,t) (7)

supplemented by the following initial and boundary conditions:

 φ(x,0)=δ(x), lim|x|→∞φ(x,t)=0, t>0 (8)

where - the diffusion coefficient, - scalar field, - the defined on positive half-line Caputo derivative of order .

The Green function of Eq. (7) with the initial and boundary conditions (8) in the time - momentum representation is equal diffusion (),diff_new () where - the Mittag-Leffler function, which is defined usually by the following series:

 Eα(z)=∞∑n=0znΓ(αn+1) (9)

In the case of real and positive the series converge for all values of the argument , thus the Mittag-Leffler function is an entire function.

There is the simple and universal technique to transform the stochastic equation  (1), (2), (8) to a field theory by doubling the number of fields double_field (). It yields an explicit form of action functional , where is a new two-component field. We plan to generalise this technique on the fractional derivative problem. Note, that the translational invariant perturbation theory with zero condition for , if is considered in critical dynamics, than time integration is performed on the entire axis in all terms. The initial condition (8) means, that integration is performed on the values only.

We will consider the following generalization of Eq. (1)

 c0Dαtφ=λV(φ)+F (10)

with a non-linear potential of the nonlinearity degree :

 V(φ)=−(−Δ)σ/2φ−τ0φ−g0φm/m! (11)

with the initial and boundary conditions

 lim|x|→∞φ(x,t)=0, φ(x,−∞)=0 (12)

and the conditions on orders of derivatives:

 0<α<1,  0<σ<2 (13)

and we assume the positivity of temperature and coupling constants: .

The power of correlation function (2) remains the same and it is equal , because in the proof of static and dynamic theory consistency the condition is used Ant_new (). It will be proved later. In the case of the Cauchy problem (8) the equilibrium distribution is realized only in the asymptotic limit , in which there is no dependence on time and on the initial data.

The potential from (10) can be written as , where the static action functional is

 ¯S(φ)=−14P.V.∫Rd×Rd(φ(x)−φ(y))2∥x−y∥d+σdxdy−∫Rd(τ02φ(x)2+g0(m+1)!φ(x)m+1)dx (14)

in the - dimensional coordinate space with coupling constant . For proof of the statement it is enough to write the difference and to take into account of the symmetry with respect to values and in (14). It’s important, that the first term in (14) is nonlocal, i.e. which is not polynom or function of the field or its derivative evaluated at a single point in the space. This reflects physically the existence of a long-range interaction in the system, and confirms the choice of operator generalization of the spatial derivative (6). Near a critical point all interactions are long range, it is confirmed by an experimental data.

Application of the renormalization group method proposes the transforming of some parameters on renormalized. The non-renormalized parameters are marked by the subscript ”0” to distinguish it from corresponding renormalized. The functional (14) at is nonlocal generalization of the Ginzburg-Landau functional, in the field theory terms it is the massive model with mass .

For the renormalization of Eq. (10) we will use the theorem of equivalence of stochastic dynamic and quantum field theory with two-component field with the main field and the auxiliary field double_field (). In the proof of this theorem assumption about just first-order of time derivative was not used. It was required only linearity of time-dependent operator. Therefore Eq. (10) is equivalent to field - theoretic model with action

 S(Φ)=∫Rdddx+∞∫−∞dt(λ0φ′φ′+φ′(−c0Dαtφ+λ0V(φ))) (15)

where . For the Cauchy problem (8) the action functional is Ant_new ():

 S(Φ)=∫Rdddx+∞∫0dt(λ0φ′φ′+φ′(−c0Dαtφ+λ0V(φ)+δ(x)δ(t−t′))) (16)

that is reduced to adding to the action of term ,since always . Statistical correlation functions (Green functions) are defined by functional average with weigh (we include in the usual minus sign in the argument ). Further we will work directly with the field - theoretical model (15). We are concerned with the restriction of parameters , allowing to apply the renormalization group method.

The asymptotics of correlators and other quantities at with already the renormalized parameter is called the critical asymptotics main_book_c (). The physical meaning of this parameter is the deviation of the critical temperature: . Our model at , , transforms to the model A, where unique non-trivial critical asymptotic is dependence of relaxation time on . It is determined by the critical exponent and has the form . Other critical asymptotics coincide with those in the static .model. For arbitrary , and it is false. In following section the difference between statics and dynamics for the field - theoretical model (15) with fractional derivatives for arbitrary vertex degree will be shown.

## 3 Determination of propagators

Standard Feynman diagram method with vertex and bare propagators is corresponded to action (15). These propagators are found by a representation of the quadratic (called ”free”) term of the action

 S0(Φ)=∫Rdddx+∞∫−∞dt(λ0φ′φ′+φ′(−c0Dαtφ−λ0(−Δ)σ/2φ−λ0τ0φ)) (17)

as the integral of a quadratic form with a symmetric operator matrix :

 S0(Φ)=−12∫Rdddx+∞∫−∞dtΦKΦ (18)

where . Then is the translationally invariant matrix of functions such that , where is the identity matrix. Using integration by parts rule for fractional derivative with respect to , we obtain from (17) the following matrix expression of matrix in the momentum representation (let ):

 (0ctDα0+Ξc0Dαt+Ξ2λ0) (19)

where is right Caputo derivative defined as

 ctDαaf(t)=(−1)nΓ(n−α)∫atf(n)(τ)dτ(τ−t)α+1−n (20)

We represent as

 (G11(x−x′,t−t′)G12(x−x′,t−t′)G21(x−x′,t−t′)0) (21)

where the functions and called propagators are sought in the class of functions vanishing at . For correctness of the iteration procedure for the equation (10) and respectively the diagram technique it is also necessary, that the condition of stability at is complied. Typically, the propagator is normalized to delta - function at coinciding times, and the requirement of delay corresponding to the physical principle of causality is imposed main_book_c (); double_field (). It can be expressed by

 G12(x−x′,t−t′)={[]rlδ(x−x′) if t=t′+00 if t

From this we see that to find the propagator we can use the Laplace transform in the variable to the variable and the Fourier transform in the variable to the variable . For convenience, different representations of propagators differ in this text by their arguments. Then the equation with (19) and (21) - (22) can be rewritten as follows at :

 sαG12(k,s)−sα−1G12(k,+0)+ΞG12(k,s) (23)

We use the property of the Mittag-Leffler function for :

 ∫∞0e−stEα(utα)dt=sα−1sα−u (24)

We finally obtain from (22) - (24):

 G12(t−t′,k)=θ(t−t′)Eα(−Ξ(t−t′)α) (25)

Similarly, we obtain the advanced propagator:

 G21(t−t′,k)=θ(t′−t)Eα(−Ξ(t′−t)α) (26)

Note, that the propagator (25) coincides with solution of the Cauchy problem (7), supplemented by the condition . Just as in model A, is the retarded propagator and is advanced. The propagator can be uniquely determined by the convolution of functions and . From (19),(21) we obtain:

 G11(k,t)=2λ0+∞∫−∞G12(k,t−t′)G21(k,t′)dt= (27) =2λ0+∞∫−∞θ(t−t′)θ(−t′)Eα(−Ξ(t−t′)α)Eα(−Ξ(−t′)α)dt= (28) =2λ0⎛⎜⎝θ(−t)t∫−∞Eα(−Ξ(t−t′)α)Eα(−Ξ(−t′)α)dt+θ(t)0∫−∞Eα(−Ξ(t−t′)α)Eα(−Ξ(−t′)α)dt⎞⎟⎠= (29) =2λ0+∞∫0Eα(−Ξt′α)Eα(−Ξ(t′+|t|)α)dt= (30) =2λ0Ξ−1/α+∞∫0Eα(−t′α)Eα(−(t′+|t|Ξ1/α)α)dt (31)

Usually the propagators and are derived in the frequency - momentum representation. If is fractional, the time derivative is replaced by factor , this factor fixes a single-valued branch. This is a well-known problem of non-physical poles separation. In our view it is more convenient to use the - representation.

## 4 Renormalization of field theoretical model in one-loop approximation

### 4.1 The analysis of scale invariance

We consider in this section the more general class of models with power-law nonlinearity :

 S(Φ)=S0(Φ)−∫Rdddx+∞∫−∞dtg0λ0φmm! (32)

It is convenient to do stretching variables in the auxiliary field with . Than the action (32) takes the form:

 S(Φ)=∫Rdddx+∞∫−∞(c0φ′φ′+φ′(−c0c0Dαtφ−(−Δ)σ/2φ−τ0φ−g0φmφ′m!)) (33)

We will consider the theory in the coordinate space of dimension .Further it is necessary to analyse scaling dimensions. We introduce the definition of two independent canonical dimensions: the momentum dimension , the frequency dimension and total for an arbitrary value Ant_vas (). By definition, , and dimensions of other quantities in (15) are found requiring dimensionless of each term in the action. From this follows, that scaling dimension of integration over all space and time is equal , scaling dimension of time derivative is , the scaling dimension of spatial derivative is . Then the system of equations, expressed dimensionless of the action (15) is

 μc0+2μφ′=αd+σ (34) μc0+μφ+μφ′+ασ=αd+σ μφ+μφ′+ασ=αd+σ μφ+μτ0+μφ′=αd+σ μφ′+μg0+mμφ=αd+σ (35)

Considering jointly the second and third equations in (35) we get , from third and fourth we obtain . We obtain immediately from first equation in (35) dimension of the auxiliary field . Dimension of the main field is obviously . Finally, the fifth equation follows .

Further, the theory is considered in the space, where the coupling constant becomes dimensionless. In this case existing divergences in correlators, if the condition of multiplicative renormalizability is complied, could be manifest in the form of poles at the deviation of the space dimension . This space dimension is called logarithmic. In our case

 d∗=σ(2mm−1−1α) (36)

Despite the possibility of analytic continuation of diagrams in the region , we think, that it is not correspond to the physical meaning of the problem. Equation  (36) clarifies restrictions on parameter as condition on positiveness of spatial dimension. Considering  (36), they become

 m−12m<α<1 (37)

This inequality (37) along with the condition of the fractional representation of the Laplacian as the principal value of the integral operator (4) and (13) is conditions for the applicability of the quantum-field renormalization group method to the equation (10). Hence we see as increasing degree of nonlinearity in the action narrows the range of permissible . The equation (36) expresses the relation between the dimension of the coordinate space and the orders of derivatives and . This provides a self-consistency of theoretical-field model (32). From inequality implies that for the usually considered range always satisfies (37).

Now for applying the renormalization group method in the space dimension it is necessary to prove the multiplicative renormalizability of the theory Ant_vas (). The form of required counterterms is found using scaling analysis of 1-irreducible Green functions. Such functions with external legs have scaling dimension , where is field scaling dimension. The divergence is determined by the total canonical dimension : the diagram has surface divergence, if in logarithmic theory is integer non-negative number. In our case at we find from (35), (36)

 δ(m−1)σα=2m−Nφ−mNφ′ (38)

This means that surface divergences exist only in 1-irreducible functions , and , i.e. only in the functions presented in (15).

Now we can write the renormalized action functional

 S(Φ)=∫Rdddx+∞∫−∞(Z1cφ′φ′+φ′(−Z2c c0Dαtφ−Z3(−Δ)σ/2φ−Z4τφ−Z5gMεφmm!)) (39)

with renormalization mass , renormalized parameters and relations between dimensionless (they depends on only) renormalization constants :

 Z1=Zφ′Zc Z2=Z1/2φ′Z1/2φZc Z3=Z1/2φ′Z1/2φ Z4=Z1/2φ′Z1/2φZτ Z5=Z1/2φ′Zm/2φZg (40)

It is known, that in model A there is a single new renormalization constant (compared with the static case). Equality of other constants follows from uniformity of Schwinger equation for static and dynamic generating functionals. The proof of this is based on , where is the renormalized static functional.

 ¯S(φ)=−¯Zφ14P.V.∫Rd×Rd(φ(x)−φ(y))2∥x−y∥d+σdxdy−∫Rd(¯Zτ¯Zφτ2φ2+¯Zg¯Z(m+1)/2φgMε(m+1)!φm+1)dx (41)

In general case we have following

###### Theorem 1

The equality of the renormalization constants (41) and (39)

 Zφ=Zφ′=¯Zφ, Zg=¯Zg, Zτ=¯Zτ (42)

holds if and only if .

The proof is constructed like model A, taking into account the fact that the logarithmic dimension of the static action functional (14) is

 d∗stat=σm+1m−1 (43)

Obviously, the coincidence of the logarithmic dimension (43) and (36) takes place only at . Thus, all UV (at large momentum) divergences manifest themselves as poles at in the renormalization constants . Further, standard renormalization group equations expressed the renormalization invariance are written. We introduce the solution of Eq. (10) as follows at :

 G(x,t|e0)=∫Dφ′∫Dφφ(x,t)exp(S(φ′,φ)) (44)

Here the normalization constant is included into the differential .

The condition of multiplicative renormalizability implies the relation for the corresponding Green functions in Eq. (44). We use to denote the differential operation for fixed and operate on both sides of this equation with it. This gives the basic RG equation :

 [DM+β(g)∂g−γg]GR(e,M)=0, Dx≡x∂x (45)

where the anomalous dimension in using the minimal subtraction scheme (MS) is expressed in terms of the renormalization constant : and doesn’t include poles at . We need to further analyse the expression for the Gell-Mann-Low function in terms of the anomalous dimension of the coupling constant :

 β(g)=−g(ε+γg(g)) (46)

The anomalous dimension of an arbitrary value expressed in terms of the corresponding renormalization constant as .

Obviously, that only as and the logarithmic space dimension of the dynamic theory coincides with the static case, we can use theorem for the coincidence of all renormalization constants excluding and accept behaviour of the Gell-Mann-Low function of the static model Ant_vas (). In the general case of the dynamic problem (15) we can not do it.

### 4.2 Calculation of the one-loop diagrams

Now we consider the case . In one-loop approximation there is only one diagram (Fig. 1) , which contribute the ordinary term in renormalization constants: ,. We can calculate it in the MS-scheme at the null external momentum and the null external frequency. The condition is equivalent to the equality of time arguments of propagators. The pole part of this diagram is denoted as : .

In MS scheme only the function will interest us. For its calculation in diagram all external momentum are supposed zero. The diagram will equal:

 Γφ′φ3=∞∫0dt∞∫0dkkd∗−ε−1G11(k,t)G12(k,t) (47)

where the logarithmic dimension is defined by  (36). Also we omit factors independent on and in the diagram. The final factor is determined from a compliance with the static case. Set in (47) (25) and (31), we can submit this as an integral:

 Γφ′φ3=∞∫0dt∞∫0dkkd∗−ε−1Eα(−Ξtα)∞∫0dτEα(−τα)Eα(−(τ+tΞ1/α)α) (48)

Replacing , we then obtain the product of two integrals

 Γφ′φ3=2λ∞∫0dkkd∗−ε−1Ξ2/α∞∫0dt∞∫0dτEα(−tα)Eα(−τα)Eα(−(t+τ)α) (49)

The integral over the momentum space is now

 ∞∫0dkkd∗−ε−1Ξ2/α=τ1σ(d∗−ε−1)−1αλ−2α∞∫0dyy(d∗−ε)/σ−1(y+1)2/α= τ1σ(d∗−ε−1)−1αλ−2αΓ(2α−d∗σ+εσ)Γ(d∗σ−εσ)Γ(2α)= τ1σ(d∗−ε−1)−1αλ−2αΓ(3α−3+εσ)Γ(3−1α−εσ)Γ(2α) (50)

and the diagram (48) is equal

 Γφ′φ3=τ1σ(d∗−ε−1)−1αλ−2αΓ(3α−3+εσ)Γ(3−1α−εσ)Γ(2α)J(α) (51)

where we denoted

 J(α)=∞∫0dt∞∫0dτEα(−tα)Eα(−τα)Eα(−(t+τ)α) (52)

In particularly at   and .

The expression (50) has a simple pole in at and at . However, the situation is forbidden by the condition (37). Therefore at and we have . In a range the expression (50) is regular, thus . It is convenient to construct the perturbation series of the coupling constant , where - surface area of the - dimensional sphere: main_book_c (). Than in the case the renormalization constant will be regular in the one-loop approximation. Hence, if

 γg(g′)=γ(1)gg′+O(g′2) (53)

then . But in the case we conclude

 γ(1)g=Cσ (54)

where is a constant which is not depend on . It is known, that in the model A at . Finally from (46) and (53),(54) we conclude

 β(g′)=−g′ε+32σg′2 (55)

The important consequence of the formula (55) is the existence of the IR stable point of the Gell-Man-Low function . This fact confirms the critical scaling at in generalized model A.

## 5 Conclusion

We applied ÐµÑÑ field theoretic renormalization group tool to the stochastic fractional derivative nonlinear equation (10). In principle, we could realize this procedure even for the nonstochastic Cauchy problem Ant_new (), but it is important for us to demonstrate a possibility of the MSR formalism application to fractional processes. Our work represents a generalization of a critical dynamics research observed in the model A. Inclusion of fractional-order derivatives of with respect to time and of with respect coordinates to the model leads to some difficulties.

Replacing the standard Laplacian by the fractional analogue leads to a nonlocal both action functionals: static and dynamic. That is why the propagators are sought in the momentum representation, in which the action is local. There are not other difficulties due to the substitution apart a nonlocality of action, and the generalization is trivial. The case is called superdiffusion.

Propagators of our model at are expressed in terms of the Mittag-Leffler function depending on the complex parameter . The propagator (31) has a complex integral representation for multi-loop calculations. This is due to the fact that the semigroup property of the Mittag - Leffler takes place only at . In this case the Mittag - Leffler function coincides with the exponential function.

We prove the multiplicative renormalizability of the model with the nonlinearity of the general form and found its logarithmic dimension (36). In the physically interesting range the logarithmic dimension is always positive.

One application of the renormalization group method to the theory of phase transitions is the establishment of scaling behaviour in the infrared asymptotic region . A necessary condition for this is the fact that the Gell-Mann-Low function has a fixed point: . From the one-loop calculation we can see, that such situation is realised with the restrictions (37) only for the superdiffusion . For the subdiffusion we can not assert something specific.

Accordingly if and the spatial dimension is less than , then in the systems controlled by the equation (10-12) the critical scaling is predicted by us.

## 6 Acknowledgements

This research is supported by the Chebyshev Laboratory (Department of Mathematics and Mechanics, St. Petersburg State University) under RF Government grant 11.G34.31.0026

## References

• (1) M. B. Isichenko, Rev. Mod. Phys. 64, 961 (1992)
• (2) G. Falkovic and K. R. Sreenivsan, Phys. Today 59(4), 43 (2006)
• (3) V. E. Tarasov, G. M. Zaslavsky, Physica A, 368:2 (2006), 399-415
• (4) Thermodynamics: An Engineering Approach ((Fourth Edition) ed.). McGraw-Hill. 2002. pp. 824.
• (5) De Dominicis C., Brezin E., Zinn-Justin J., Phys. Rev., B12:11 (1975), 494-495
• (6) Hohenberg P. C., Halperin B. I., Rev. Mod. Phys., 49:3 (1977), 435-479
• (7) A.N. Vasiliev, Functional Methods in Quantum Field Theory and Statistical Physics, Gordon and Breach, New York, 1998
• (8) J. Zinn-Justin, Quantum Field Theory and Critical Phenomena, Oxford Univ. Press, New York, 1989
• (9) E. Lutz, Fractional Langevin equation, Phys. Rev. E 64 (2001) 051106-1-051106-4
• (10) O. P. Agrawal, Solution for a fractional diffusion-wave equation defined in a bounded domain, Nonlinear Dynamics 29 (2002), 145-155
• (11) Antonov, N. V, Field-theoretic renormalization group for a nonlinear diffusion equation, Physical Review E, 66:4 (2002), 046105
• (12) E. Barkai, Fractional Fokker-Planck equation, solution, and application, Phys. Rev. E 63 (2001)
• (13) Renormalization of tracer turbulence leading to fractional differential equations, Phys. Rev. E 74 (2006)
• (14) N. V. Antonov, A. N. Vasiliev, Critical dynamics as a field theory, Teoret. Mat. Fiz., 60:1 (1984), 59-71
• (15) J Bonart, L F Cugliandolo and A Gambassi, Journal of statistical mechanics-theory and experiment, P01014, 2012, Critical Langevin dynamics of the O(N)-Ginzburg-Landau model with correlated noise
• (16) A. A. Kilbas, H. M. Srivastava, J. J. Trujillo, Theory and Application of Fractional Differential Equations, North-Holland Math. Stud., 204, Elsevier, Amsterdam, 2006
• (17) Gorenflo, R. and Mainardi, F. (1998), Random walk models for space-fractional diffusion processes, Fractional Calculus and Applied Analysis, 1, 1677-191.
• (18) Hanyga, A. (2001), Multi-dimensional solutions of time-fractional diffusion-wave equations, Proc. R. Soc. London A.
• (19) Martin P. C., Siggia E. D., Rose H. A., Phys. Rev., A8:1 (1973), 423 - 437
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