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ORIGINAL RESEARCH article

Front. Phys., 15 January 2024
Sec. Statistical and Computational Physics
This article is part of the Research Topic Advances in Nonperturbative Approaches: Methods, Algorithms, and Applications View all articles

Original and modified non-perturbative renormalization group equations of the BMW scheme at the arbitrary order of truncation

  • 1Laboratory of Semiconductor Physics, Institute of Technical Physics, Faculty of Materials Science and Applied Chemistry, Riga Technical University, Riga, Latvia
  • 2Institute of Science and Innovative Technologies, University of Liepaja, Liepaja, Latvia
  • 3The MS2 Discovery Interdisciplinary Research Institute, Wilfrid Laurier University, Waterloo, ON, Canada
  • 4BCAM - Basque Center for Applied Mathematics, Bilbao, Spain

We consider the non-perturbative renormalization group (RG) equations, obtained as approximations of the exact Wetterich RG flow equation within the Blaizot–Mendez–Wschebor (BMW) truncation scheme. For the first time, we derive explicit RG flow equations for the scalar model at the arbitrary order of truncation. Moreover, we consider original, as well as modified, approximations, used to obtain a set of closed equations. We compare these equations at the s = 2 order of truncation with those recently derived in J. Phys. A: Math. Theor. 53, 415002 (2020) within a new truncation scheme and find a striking similarity. Namely, the first-order equations of the latter scheme, those of the original BMW scheme, and those of the modified BMW scheme (at s = 2) differ only in one term. We solved these equations by a recently proposed and tested method of semi-analytic approximations. Thus, the critical exponents η, ν, and ω were evaluated, recovering also the known results of the original BMW scheme. In addition, we estimated the subleading correction-to-scaling exponent ω2 for the three equations considered. To the best of our knowledge, this exponent has not yet been extracted from the Wetterich equation beyond the local potential (the zeroth order) approximation. Our current estimate for the 3D Ising model is ω2 = 2.02 (40), where the error bars include the expected truncation error in the BMW scheme.

1 Introduction

The renormalization group (RG) method is one of the most widely used approaches in the analysis of critical phenomena [15]. Here, we consider the non-perturbative RG approach [69], focusing on the Wetterich equation and its approximation schemes, developing further the research initiated in [10].

The functional renormalization group approach, which is at the heart of models such as the Wetterich and the Polchinski equations, provides an appropriate framework for the analysis of a range of central problems in many areas, including quantum systems, Yang–Mills theories, and statistical physics, see, e.g., [11], for a review. The Wetterich and Polchinski equations of the functional renormalization group belong to the so called non-perturbative RG equations. They have been successfully applied to many particular systems, including the Ginzburg–Landau model [1018], quantum models and quantum gravity [1930], and the tensorial group field theory [31]. It has been applied to equilibrium, as well as out-of-equilibrium systems and critical dynamics [3234]. A recent review of all these applications is given in [35].

While the Wetterich equation itself is exact, it cannot be solved exactly. Approximate closed equations are obtained from it, applying certain truncation schemes for the effective action. The local potential approximation (LPA) is a widely known lowest-order approximation, which is traditionally improved step by step by the derivative expansion (DE) [9,14]. As alternative truncation schemes, the vertex expansion [14], the BMW scheme [17], and the recent scheme proposed in [10] can be mentioned. In distinction to the derivative expansion, which relies on the small momentum (wave vector magnitude) approximation, the latter two schemes preserve the full momentum dependence.

In this paper, we report the results of a significant further development of the BMW scheme for the scalar model, deriving explicit equations for calculations at the arbitrary order of truncation within this scheme, as well as proposing useful modifications of the original BMW scheme. Moreover, we established an intrinsic link between the equations of the BMW scheme and those of the recent scheme proposed in [10] at the first order of truncation. A recently developed method of semi-analytic approximations [36] was used to solve these equations.

The usefulness of our new developments is demonstrated in example calculations for the scalar model in three dimensions, where we evaluate the critical exponents, including the subleading correction-to-scaling exponent ω2, for which quite limited results are available in the literature. Apparently, such results for ω2 are obtained here for the first time from the Wetterich equation beyond the LPA, and we found only a relatively old estimate ω2 = 1.67(11) from the Polchinski equation at the O2 order of DE [37]. The RG estimations of the correction-to-scaling exponents have a fundamental significance as a crucial test of consistency with the conformal field theory (CFT) [38,39]. The RG estimate of ω2 mentioned here does not reveal such a consistency, since ω2 = 3.8956(43) is expected from the CFT [39,40]. We will return to this issue in the summary of our current results at the end of this paper.

Our paper is organized as follows. The Wetterich equation is reviewed in Sec. 2, and the BMW scheme of its truncation is reviewed in Sec. 3. Our new developments of the BMW scheme, including the equations at the arbitrary order of truncation, are presented in Sec. 4 with details of the derivation being given in Supplementary Material SA1. The comparison of equations of the BMW scheme with those derived in [10] is made in Sec. 5, providing the dimensionless form of these equations in Sec. 6. The results of numerical calculations are collected in Sec. 7. The summary of results and outlook, pointing to potential further applications and developments, are provided in Sec. 8.

2 Wetterich equation

In statistical physics, equilibrium systems of interacting particles are routinely described by the action S = H/(kBT), where H is the Hamiltonian and kB is the Boltzmann constant. A basic example is the Ising model with S [σ] = −β∑ijσiσjh∑iσi, where σi = ±1 is the spin variable at the ith lattice site, ⟨ij⟩ denotes the pairs of nearest neighbors, β is the coupling constant, and h is the normalized (divided by kBT) interaction energy between a spin with σi = ±1 and the external field. Another simple example is the φ4 model with S[φ]=ddxαφ2+β(φ2)2+γ(φ)2, where α, β and γ are the expansion coefficients for the density of S with a continuous order parameter φ(x), which depends on the coordinate x in the d-dimensional space. In the simplest case, it is scalar, but can also be an n-component vector. The scalar φ4 model is known to belong to the Ising universality class, which means that the behavior of φ4 and the Ising models near the phase transition point is described by the same critical exponents.

It is convenient to use the wave vector representation of the action S[φ] via the Fourier transformation φ(x) = Ω−1/2 qφ(q)eiqx, where Ω is the volume of the system. The critical behavior is related to the long-wavelength (infrared) or small-|q| fluctuations [3], but one should also control the ultraviolet fluctuations. A point here is that S[φ] might be ill-defined without an appropriate upper or ultraviolet cut-off in the wave vector (momentum) space. In the φ4 model, one needs to introduce such a cut-off, e.g., by setting φ(q) ≡ 0 at q > Λ (where q = |q|) to avoid ultraviolet divergences in various calculations, e.g., in the calculation of ⟨φ2⟩. The cut-off parameter Λ refers to the shortest or “microscopic” length scale ∼ π/Λ of the model, like the lattice constant in the Ising model.

The general idea of the RG method is to look at a system on different length scales. In the Wetterich functional RG approach [6,9], this idea is realized by introducing an infrared running cut-off scale k, in such a way that fluctuations with qk are suppressed, those with qk being practically unaffected. For this purpose, the action is modified as S[φ] → S[φ] + ΔSk[φ] [9], where

ΔSkφ=12ddq2πdi=1NφiqRkqφiq.(1)

Here, φ is an N-component vector with components φi, whereas Rk(q) is the infrared cut-off function with properties Rk(q) → 0 at k → 0 and Rk(q) → at k for fixed q. A simple choice, proposed in [6,9], is

Rkqq2eq2/k21.(2)

For q2k2, this cut-off behaves as Rk(q) ∼ k2. It means that the Fourier modes φi(q) with small momenta q < k acquire a weight factor or effective mass ∼ k included in the term (1). This additional mass acts as an effective infrared cut-off for these low-momentum modes. More precisely, this effect is essential in vicinity of the critical point, where Rk(q) smoothly cuts off the critical infrared fluctuations at a finite k. The cut-off function (2) tends (exponentially fast) to zero at large q/k values; therefore, the high-momentum modes with q/k are not disturbed by ΔSk[φ].

Further on, an averaged order parameter ϕ(x) = ⟨φ(x)⟩ is introduced, where the averaging is performed over φ(x) in the presence of external sources J(x). The averaged field ϕ(x) depends on J(x), and this dependence is affected by k, i.e., ϕ = ϕk(J). There exists also the inverse relation in the sense of the Legendre transformation J = Jk(ϕ). The effective average action Γk[ϕ] is considered as a functional of ϕ according to the definition

Γkϕ=lnZkJ+ddxiJiϕiΔSkϕ,(3)

where Ji are the components of the vector J(x) and Zk is the partition function

ZkJ=DφexpSφΔSkφ+ddxiJiφi.(4)

In (3), J(x) is the Legendre transform of ϕ(x), i.e., J = Jk(ϕ).

An exact RG flow equation, describing the variation of Γk[ϕ] with the infrared cut-off scale k, has been obtained in [6]. A detailed non-perturbative derivation has been later reported in [9]. This equation, called the Wetterich equation, reads

kΓkϕ=12TrΓk2ϕ+Rk1kRk.(5)

In this equation, k decreases toward k = 0, starting from some initial value k0. Thus, it generally allows describing the physics of various models with various choices of the order-parameter field by smoothly interpolating between different length scales.

Starting with k0 = Λ (as in our calculations), only the fluctuations at the microscopic length scale q ∼Λ are properly taken into account in the initial stage of the integration of RG flow Eq. 5. Fluctuations of the original model (where ΔSk = 0) with longer and longer wavelengths are gradually restored as k → 0. At k = 0, all fluctuation modes are included so that Γk=0 [ϕ] is the effective action of the original model, defined by (3) without the term ΔSk [ϕ]. Another possibility, discussed in [35], is to choose k0 ≫Λ. In this case, all fluctuations are frozen at the beginning (since the original model contains only the modes with q < Λ, and these are suppressed at k ≫Λ) and Γk0[ϕ]=S[ϕ] holds as in Landau’s mean-field theory of phase transitions.

For the O(N) model, ϕ(x) is a vector with components ϕj(x), where j = 1, … , N. It is convenient to consider (5) in the space of wave vectors q, where

ϕjx=Ω1/2qϕjqeiqx,(6)
ϕjq=Ω1/2ϕjxeiqxdx,(7)

Ω being the volume of the system, for which periodic boundary conditions are assumed. The wave vectors are restricted by the upper cut-off, i.e., q < Λ. In this representation, the quantity Γk(2)[ϕ] is a matrix with elements

Γk2ijq,q=δ2Γkϕδϕiqδϕjq.(8)

For the discrete wave vectors in (6), the cut-off function Rk is represented as [10]

Rk,ijq,q=Rkqδijδq,q.(9)

The choice of Rk(q) is not unique, and several possibilities have been considered in [11,18]. For simplicity, here we have limited our choice to

Rkq=αZkq2eq2/k21,(10)

traditionally used in many investigations [9,14,17], where Zk is a renormalization constant and α is an optimization parameter. This cut-off function coincides with (2) and, thus, has the required properties discussed before. It allowed us to compare the results with those of [17], where the same cut-off function was used.

3 The BMW scheme of truncation

Here, we review the BMW truncation scheme for the scalar model, considered in detail in [17], noting that the N-component case has also been considered there in the Appendix. In the BMW truncation scheme, one considers the s-point functions Γk(s)(q1,q2,,qs;ϕ) as the Fourier transforms of δsΓk [ϕ]/(δϕ(x1)δϕ(x2)⋯δϕ(xs)). We found it convenient to use an equivalent definition in the wave vector space, i.e.,

Γksq1,q2,,qs;ϕ=Ωs21δsΓkϕδϕq1δϕq2δϕqs,s2.(11)

The basic idea of this truncation scheme is to consider first a hierarchy of exact equations for these s-point functions, obtained by applying the functional derivatives to (5). Approximate closed equations are then obtained, using certain approximations of the higher order functions (at orders s + 2 and s + 1) by the lower-order functions (up to the order s).

For constant ϕ, one has

Γkϕ=ΩVkϕ,(12)

where Vk(ϕ) is the potential. The exact RG flow equation for it is obtained by evaluating the Wetterich equation at ϕ = const. Using the notations t = ln k, ρ=12ϕ2, and

qddq2πd,(13)

where the integration is performed over the region q < Λ, this equation reads

tVkρ=12qtRkqGkq,ϕ,(14)

where

Gk1q,ϕ=Γk2q,ϕ+Rkq(15)

is the two-point correlation function with Γk(2)(q,ϕ)Γk(2)(q,q;ϕ), evaluated at ϕ = const.

In the zeroth-order approximation (s = 0) or LPA, one sets [17]

Γk2q,ϕq2+Γk20,ϕ=q2+ϕ2Vkϕ,(16)

where the coefficient 1 at q2 corresponds to the usually assumed coefficient 1/2 at the gradient term (∇ϕ)2 in the coordinate representation of Γk [ϕ], i.e.,

ΓkLPAϕ=ddx12ϕ2+Vkϕ.(17)

Using (16), Eq. 14 becomes a closed approximate RG flow equation for the potential Vk(ϕ).

In order to obtain the equations at the s = 2 order, one considers the RG flow for Γk(2). An exact flow equation is obtained, taking two functional derivatives with respect to the field [based on (11)] in Wetterich Eq. 5 and evaluating the resulting expression at ϕ = const. It yields [17]

tΓk2p,ϕ=qtRkqGk2q,ϕ×{Γk3p,q,pq;ϕGkq+p,ϕΓk3p,p+q,q;ϕ12Γk4p,p,q,q;ϕ}.(18)

According to the original idea of the BMW truncation scheme, a closed approximate equation is obtained from this by setting the internal momenta equal to zero, i.e., q = 0, in the arguments of Γk(3) and Γk(4). Generally, this is done for Γk(s+1) and Γk(s+2) at order s. Thus, the momentum dependence of the highest-order functions is represented in a simplified approximate form, considering q as a small quantity. Using the exact formula

Γks+1pi,0;ϕ=ϕΓkspi;ϕforϕ=const,(19)

these simplified expressions for Γk(s+1) and Γk(s+2) are further reduced to the derivatives of Γk(s), thus obtaining closed equations. Equation 19 is a consequence of (11), noting that ϕ(q) = Ω1/2ϕ δq,0 holds for homogeneous field ϕ(x) = ϕ = const according to (7).

At s = 2, the equation for Γk(2)(p,ϕ) reads [17]

tΓk2=J3p,ϕϕΓk2212I2ϕϕ2Γk2,(20)

where

Jnp,ϕ=qtRkqGkp+q,ϕGkn1q,ϕ,(21)
Inϕ=Jn0,ϕ.(22)

It is important to note that Γk(2) is represented exactly as

Γk2p,ϕ=Γk2p,ϕΓk20,ϕ+ϕ2Vkϕ,(23)

keeping the term ϕ2Vk(ϕ), inherited from the zeroth-order approximation, untouched and solving the RG flow equation for the difference Γk(2)(p,ϕ)Γk(2)(0,ϕ). Moreover, it has also been suggested in [17] to separate the zeroth-order contribution q2 from this difference.

4 Equations of the BMW scheme at the arbitrary order of truncation

4.1 Exact RG flow equations for the n-point functions

Here, we derive exact RG flow equations for the n-point function at any n, from which approximate closed equations at arbitrary truncation order s are then obtained, as described in Sec. 4.3. In the following, we summarize these equations, the details of the derivation being provided in Supplementary Material SA1. For brevity, we omitted ϕ in the list of arguments of the n-point functions Γk(n), noting also that this argument is subsequently replaced by ρ = ϕ2/2 in our treatment. Thus, according to Supplementary Material SA1, for ϕ = const, we have

tΓknp1,p2,,pn=12M=1n1Mm1,m2,,mMm1++mM=njim1,,mMnqtRkq×Gkqi=1MΓk2+mipj1i,pj2i,,pjmii,Q`i,QiĜkQi,(24)

where l=1npl=0 holds, 1 ≤ min are integers, and j(i)m1,,mMn are the distributions of n integer numbers 1, 2, … , n over M boxes with m1 numbers in the first box, m2 numbers in the second box, and so on (totally n!/(m1!m2!⋯mM!) possibilities). Here, j(i) with = 1, 2, … , mi are the numbers in the ith box. We ordered them by index in such a way that j1(i)<j2(i)<<jmi(i). In addition, Ĝk(Q) is the correlation function, which is modified by the upper cut-off as

ĜkQ=GkQθΛQ.(25)

This cut-off is included here to follow a formal rigor in treating such cases, where the original action S[φ] is ill-defined without it, see Sec. 2. It influences the RG flow in the Wetterich equation only at k ∼Λ for k ≤ Λ. Therefore, it can be further omitted, considering the vicinity of the fixed point at k → 0, as it is usually performed in the literature.

For any given m1, m2, … mM at the considered n, the wave vectors Qi are defined by

Q`i=ql=iMPl,1iM,(26)
Qi=q+l=i+1MPl,1iM,(27)

where the latter sum is defined as zero for i = M (so that QM = q) and

Pi==1mipji,1iM.(28)

At i = 1, Eqs 26, 27 reduce to

Q`1=q,Q1=qP1,(29)

noting that

i=1MPi=l=1npl=0.(30)

The known Eq. 18 can be easily recovered from (24). Following notations introduced after Eq. 15 and noting that p1 + p2 = 0 holds in (24) at n = 2, we have tΓk(2)(p1) on the left-hand side of this equation at n = 2. In this case, the sum over M contains only two terms, M = 1 and M = 2. At M = 1, the next sum reduces to m1 = n = 2, and the last sum reduces to j1(1) = 1 and j2(1) = 2. It corresponds to two numbers, 1 and 2, put in a single box (i = 1, = 1, 2). These numbers are identified with j1(1) and j2(1). One has j1(1) = 1, j2(1) = 2 due to the ordering j1(1) < j2(1). Furthermore, we find Q1 = q from (27), P1 = p1 + p2 = 0 from (28), and Q`1=q from (26). Hence, M = 1 gives the contribution

tΓk2p11=12qtRkGk2qΓk4p1,p1,q,q(31)

to (24), noting that Ĝk(q)=Gk(q) holds, since 0 < q < Λ.

At M = 2, the second sum reduces to m1 = m2 = 1 for n = 2, whereas the following sum comprises two cases: 1) j1(1) = 1, j1(2) = 2 and 2) j1(1) = 2, j1(2) = 1 (we have i = 1, 2 and = 1). In the first case, we obtain (using Eqs 2628, where p1 + p2 = 0) P1 = p1, P2 = p2, Q`1=q, Q1 = q + p2, Q`2=qp2, and Q2 = q. The second symmetric case is obtained from the first one via p1p2. Hence, M = 2 gives the contribution

tΓk2p12=12qtRkqGk2qΓk3p1,q,q+p2Ĝkq+p2Γk3p2,qp2,q+Γk3p2,q,q+p1Ĝkq+p1Γk3p1,qp1,q],(32)

where Ĝk(q)=Gk(q) is used as in (31). This expression is modified by setting p2 = −p1. Furthermore, the replacement q → −q is performed in the first line of (32) (owing to the symmetric integration region |q| < Λ) followed by the change of the sign for the arguments of Gk and Ĝk (since Gk(Q) = Gk (−Q)). In the second line of (32), the last two arguments of Γk(3) are exchanged, using the symmetry of the n-point functions. After these replacements, it becomes evident that two terms in the square brackets give equal contributions, and (32) reduces to

tΓk2p12=qtRkqGk2qΓk3p1,q,qp1Ĝkq+p1Γk3p1,q+p1,q.(33)

Equation 18 is obtained by summing up both contributions (31) and (33), exchanging the last two arguments of Γk(4) (using the symmetry), omitting the upper cut-off for Ĝk(q+p1), redenoting p1p, and reintroducing the argument ϕ, which is skipped for brevity.

If Γk(n) is an analytic function of ϕ2 for even n, then it is representable as ϕ multiplied by an analytic function of ϕ2 for odd n, as it follows from (19). Therefore, we introduce the new n-point functions

Γ̂kn=DefΓkn,for evenn,ϕ1Γkn,for oddn,(34)

which are all analytic functions of ρ = ϕ2/2. Substituting these new functions in RG flow Eq. 24, we easily obtain

tΓ̂knp1,p2,,pn=12M=1n1Mm1,m2,,mMm1++mM=njim1,,mMnqtRkq×2ρμnm1,,mMGkqi=1MΓ̂k2+mipj1i,pj2i,,pjmii,Q`i,QiĜkQi,(35)

where

μnm1,,mM=Nm1,,mM/2for evenn,Nm1,,mM1/2for oddn,(36)

where N(m1,,mM) is the number of odd mi in the sequence m1, m2, … , mM. Due to the condition m1 + m2 + ⋯ + mM = n, N is even for even n and odd for odd n. Consequently, μn is always a non-negative integer number.

4.2 Some useful relations

In this section, we introduce some exact relations, which are useful for building up the approximation schemes in Sec. 4.3.

First, we consider the structure of arguments of the highest-order term Γk(n+2) in Eq. 24 for Γk(n). This term appears only at M = 1, m1 = n, and there is only one j(i) distribution possible in this case, i.e., i = 1, j(1) = with 1 ≤ n. Since i = 1, we have Q1 = q and Q̀1=q according to (29), noting that P1 = p1 + ⋯ + pn = 0 holds for this j(i). Thus, Eq. 24 contains Γk(n+2) in the form of Γk(n+2)(p1,p2,,pn,q,q).

Similarly, we consider the arguments of the Γk(n+1) function, contained in the equation for Γk(n). The (n + 1)-point function appears at M = 2 in two subcases: 1) m1 = 1, m2 = n − 1 and 2) m1 = n − 1, m2 = 1. Using relations (26)(29), we easily establish that Γk(n+1) is contained in the forms of Γk(n+1)pj1,pj2,,pjn1,q=1n1pj,q and Γk(n+1)pj1,pj2,,pjn1,q,q=1n1pj, where all possible sequences of indices j appear, which are obtained by skipping one of the numbers in the sequence 1, 2, … , n.

As the next step, we consider the exact relations

Γkn+2p1,p2,,pn,q,q=ϕ2Γknp1,p2,,pn+Δ2,kn+2p1,p2,,pn,q,q,(37)
Γkn+1pj1,pj2,,pjn1,qpj,q=ϕΓknpj1,pj2,,pjn1,pj(38)
+Δ1,kn+1pj1,pj2,,pjn1,qpj,q,()

following from (19), where pj=1n1pj and

Δ2,kn+2p1,p2,,pn,q,q=DefΓkn+2p1,p2,,pn,q,qΓkn+2p1,p2,,pn,0,0,(39)
Δ1,kn+1pj1,pj2,,pjn1,qpj,q=DefΓkn+1pj1,pj2,,pjn1,qpj,q(40)
Γkn+1pj1,pj2,,pjn1,pj,0.()

Using these relations, Γk(n+1) and Γk(n+2) can be expressed by ϕΓk(n), ϕ2Γk(n), Δ1,k(n+1), and Δ2,k(n+2) in the equation for Γk(n), noting that (38) holds for arbitrary wave vectors, and the arguments can be exchanged. In particular, one can exchange the last two arguments and replace q → −q to obtain the necessary relation for Γk(n+1)pj1,pj2,,pjn1,q,q=1n1pj.

In the following, we derive such relations for the n-point functions Γ̂k(n+2) and Γ̂k(n+1), expressed by the derivatives with respect to ρ. Using the definitions (34) and ρ = ϕ2/2, we obtain from (37) to (38) the desired equations:

Γ̂kn+2p1,p2,,pn,q,q=H2nΓ̂knp1,p2,,pn+Δ̂2,kn+2p1,p2,,pn,q,q,(41)
Γ̂kn+1pj1,pj2,,pjn1,qpj,q=H1nΓ̂knpj1,pj2,,pjn1,pj(42)
+Δ̂1,kn+1pj1,pj2,,pjn1,qpj,q,()

where H1(n) and H2(n) are the differential operators

H1n=ρfor evenn1+2ρρfor oddn,(43)
H2n=ρ+2ρρ2for evenn3ρ+2ρρ2for oddn(44)

and the quantities Δ̂j,k(n+i) are defined as

Δ̂2,kn+2p1,p2,,pn,q,q=DefΓ̂kn+2p1,p2,,pn,q,qΓ̂kn+2p1,p2,,pn,0,0,(45)
Δ̂1,kn+1pj1,pj2,,pjn1,qpj,q=DefΓ̂kn+1pj1,pj2,,pjn1,qpj,q(46)
Γ̂kn+1pj1,pj2,,pjn1,pj,0.

4.3 Closing approximations

Based on the relations of Sec. 4.2, we modify Eq. 35 for 2 ≤ ns to the form appropriate for making certain closing approximations. In addition, we consider two variants of such modifications.

1. The Γ̂k(n+2) and Γ̂k(n+1) functions in the equation for n = s, as well as the Γ̂k(n+2) function in the equation for n = s − 1 (at s > 2), are substituted by the corresponding expressions on the right-hand side of Eqs (41), (42) and of the symmetric to (42) with qpj,qq,qpj

2. The substitutions of Γ̂k(n+2) and Γ̂k(n+1), using Eqs (41), (42) and the symmetric to (42), are performed in each of the equations with 2 ≤ ns

In addition, the change of variable from Γ̂k(2)(q,q)Γk(2)(q) to

Δkq=Γ̂k2q,qΓ̂k20,0(47)

is performed, which means that Γ̂k(2)(q,q) is replaced by

Δkq+ϕ2Vk=Δkq+H22Vk(48)

in accordance with (23). In this case, the RG flow equation for Δk reads

tΔkp=tΓ̂k2p,ptΓ̂k20,0,(49)

with terms on the right-hand side being given in (35). Such a change of variable is meaningful, as it preserves the term ϕ2VkH2(2)Vk of the zeroth-order (LPA) approximation. One has to note that Δk has been defined in [17] by Γk(2)(q)=q2+Δk(q)+ϕ2Vk to keep explicitly also the LPA term q2. However, this choice is optional, since the RG flow equation for Δk is just the same, and it does not finally lead to a different approximation.

With the above replacements made in (35), we obtain a modified set of exact equations up to arbitrary order s. However, this set of equations is not closed because it contains the functions Δ̂1,k(s+1), Δ̂2,k(s+2) for s ≥ 2, and also Δ̂2,k(s+1) for s > 2, which are defined in terms of Γ̂k(s+1) and Γ̂k(s+2). Therefore, we consider certain closing approximations for them, proposing again two different options (a) and (b).

(a) We set Δ̂1,k(s+1)=Δ̂2,k(s+2)=0 for s = 2 or Δ̂1,k(s+1)=Δ̂2,k(s+2)=Δ̂2,k(s+1)=0 for s > 2.

(b) These quantities are approximated by their values at zero external momenta pj. Namely, we start with the approximations

Δ2,kn+2p1,,pn,q,qΔ2,kn+20n,q,q,(50)
Δ1,kn+1pj1,,pjn1,Qpj,QΔ1,kn+10n1,Q,Q,(51)

where {0}n is the string 0, … , 0 of n zeroes, from which we obtain

Δ̂2,kn+2p1,,pn,q,qH2nΔΓ̂knq,(52)
Δ̂1,kn+1pj1,,pjn1,Qpj,QH1nΔΓ̂knQ(53)

with the help of (19), (34), and the definitions of Δj,k(n+i) and Δ̂j,k(n+i). Here, Q = q is set in one case and Q = −q with exchanging the last two arguments in the symmetric case, whereas ΔΓ̂k(q) is defined by

ΔΓ̂knq=DefΓ̂kn0n2,q,qΓ̂kn0n.(54)

The closing approximations are represented by (52)(53) at n = s, as well as by (52) at n = s − 1 if s > 2.

In summary, the final closed system of equations at the arbitrary order of truncation s is represented by Eq. 14 (where we omit ϕ for brevity) with

Gkq=1/H22Vk+Δkq+Rkq,(55)

completed by explicit Eq. 35 for 2 ≤ ns, in which certain precisely defined replacements are performed. In particular, (49) is used for n = 2. In this sense, we derived an explicit closed system of equations for arbitrary s. There exist approximations with s = 0, 2, 3, 4, 5, etc., and only the order s = 1 does not exist.

We proposed four different versions of the replacements in (35), which can be numbered as 1a, 1b, 2a, and 2b, corresponding to options 1 and 2 for the exact modification of (35) and options (a) and (b) for the closing approximations used. Thus, we have four different modifications within the BMW scheme.

In fact, the original BMW scheme corresponds to 1a, since the q-dependence of Γk(s+2) and Γk(s+1) is neglected in this case, evaluating them at q = 0 (option (a)), and the n-point functions with n > 2 are not modified in any other way (option 1).

Option 2, including modifications for all n-point functions with 2 < ns, is indeed quite meaningful. Namely, in analogy with keeping the zeroth-order term H2(2)Vk untouched, it preserves at higher orders all those terms, which appear as Hi(n)Γ̂k(n) at lower orders. Hence, 2 might be a better option than 1. These options 1 and 2 represent exact modifications and, therefore, are equally good at the stage of their implementation. However, the final approximations are influenced by the specific choice. In particular, relations (41)(42) with Δj,k(n+i) defined in (45)(46) will not be satisfied exactly by approximate solutions, in general. A difference will appear because these relations for n + is are implemented in the RG flow equations in option 2, but not in option 1. These two options are indistinguishable at s = 2. In this case, we have to choose between (a) and (b) only.

In fact, choice (a) relies on the smallness of the internal momentum q when approximating Γ̂k(s+i) with i > 0, whereas (b) relies on the smallness of the external momenta pj when approximating the differences Δ̂j,k(s+i) with i > 0. Intuitively, (b) might be a better choice than (a) since the latter one reduces simply to the setting Δ̂j,k(s+i)=0. Thus, physically, a common basic feature of the original BMW scheme (a) and the modified BMW scheme (b) is that both of them rely on the smallness of some of the momenta in the closing approximation. However, a difference is that this is the internal momentum in the original scheme and the external momenta in the modified one. From this aspect, option (b) is similar in spirit to the truncation approximation used in the scheme of [10], where the internal momentum (the integration variable) in no sense is considered as being small.

From some other aspects, the versions of the BMW scheme are essentially different from the scheme of [10]. A truncation is applied directly to Γk[ϕ] in the latter scheme. Hence, one has to think how good or how well justified is the proposed specific truncation performed over an infinite set of terms or vertices contained in the exact Γk[ϕ]. It refers to any scheme, which deals with a direct truncation of Γk[ϕ]. The BMW scheme, including its current modifications, is quite different. Namely, the hierarchy of exact Eq. 24 appears in an unambiguous and natural way, and one only needs to think about an appropriate closing approximation of the highest-order n-point functions by lower order ones. The fact that this hierarchy is now explicitly written down for arbitrary n (via Eq. 24 or Eq. 35) can also be seen as an essential advantage of this scheme. According to the actual results at s = 2, discussed in the following sections, the closing approximations considered here are reasonably good, at least, as regards the critical exponents η, ν, and ω. Following the intuitive argument proposed above, we expect that the modified approximation (b) is generally better than the original one (a) since it should be better to approximate Δ̂j,k(s+i) than simply omit this term.

A quite different closing approximation for the equations at s = 2 has been proposed in Appendix B of [17]. However, our first result obtained by this approximation was unsatisfactory, i.e., η = 0 at the simplest choice p0 = ρ0 = 0 of the free parameters p0 and ρ0 introduced in [17]. Therefore, we have further skipped this version.

5 Comparison of equations at s = 2

Here, we consider in detail the truncation order s = 2. We revealed a striking similarity between the RG flow equations in the original (option (a)) and the modified (option (b)) BMW schemes at s = 2 on one side and the scheme of [10] at the first order of truncation on the other side. According to Sec. 4 in this paper and Eq. 43 (together with the related equations) in [10], we have

tΔkp=qtRkqGk2q{2ρvkρ+akp,q2Gkq+pθΛ|q+p|2ρvkρ+ak0,q2Gkq12Δkp+2ρΔkp},(56)

where

vkρ=3Vkρ+2ρVkρ(57)

and

akp,q=Δkpin the original BMW schemeΔkp+Δkqin the modified BMW scheme12Δkp+Δkq+Δkp+qin the scheme of [10],(58)

noting only that Δk and Vk correspond to 2Ψk and Uk in [10], and the primes denote the derivatives with respect to ρ. Equation 56 with the first choice in (58) coincides with Eq. 23 in [17]. Thus, the RG flow equations differ only in one term ak (p, q) in the three cases considered. This is a really striking similarity, especially if we note that the equations of [10] have been derived in a completely different way than those of the BMW scheme.

It is interesting to mention that the expression for ak (p, q) in the modified BMW scheme agrees with that in the original BMW scheme at q = 0 (since Δk (0) ≡ 0), whereas it agrees with that in the scheme of [10] at p = 0.

6 Dimensionless equations at s = 2

For the application of critical phenomena, we write the RG flow equations in a scaled (dimensionless) form, using the transformations

Vkρ=kdukρ̃,whereρ̃=Zkk2dρ,(59)
Rkq=Zkq2ry,wherey=q2/k2,(60)
Δkq=Zkq2fkρ̃;y,(61)

where Zk=limq0Δk(q)/q2|ρ=0, and

ry=αey1(62)

corresponds to (10). In addition, the dimensionless equations contain the running exponent η(k) = −d ln Zk/dt. As in [10], the above transformations led to the following RG flow equations:

tukρ̃=dukρ̃+d2+ηkρ̃ukρ̃Kd40Λ2/k2yd21ζkydyPkρ̃,y,(63)
tfkρ̃;y=ηkfkρ̃;y+ρ̃d2+ηkfkρ̃;y+2yfkρ̃;yy+Kd4fkρ̃;y+2ρ̃fkρ̃;y0Λ2/k2y1d21ζky1dy1Pk2ρ̃,y1y1Ĉkρ̃,yĈkρ̃,0,(64)

where

ζky=2y2ry+ηkyry,(65)
wkρ̃=ukρ̃+2ρ̃ukρ̃,(66)
Pkρ̃,y=wkρ̃+yfkρ̃;y+ry(67)

and

Ĉkρ̃,y=ρ̃K̃d0Λ2/k20πζky1ΘΛ2k2Yy1d21sinθd2×wkρ̃+âkρ̃;y,y12Pkρ̃,YPk2ρ̃,y1dy1dθ,(68)

where

âkρ̃;y,y1=yfkρ̃;yin the original BMW schemeyfkρ̃;y+y1fkρ̃;y1in the modified BMW scheme12yfkρ̃;y+y1fkρ̃;y1+Yfkρ̃;Yin the scheme of [10].(69)

Here, Y=y+y1+2yy1cosθ, primes denote derivatives with respect to ρ̃, except for r′(y) = dr/dy, and Θ is the Heaviside theta function. In addition, Kd = S(d)/(2π)d and K̃d=S(d1)/(2π)d, where S(d) is the surface of unit sphere in d dimensions. For convenience, we replaced the sharp upper cut-off in (68) by a smooth one, as in [36].

It should be noted that fk (0; 0) ≡ 1 holds according to the definition of Zk; therefore, η(k) is found from the condition tfk (0; 0) ≡ 0. Hence, the equation for η(k) reads

ηk=Kd4fk0;00Λ2/k2yd21ζkydyPk20,y.(70)

The dimensionless equations of [17] are recovered with the first choice in (69), whereas those of [10] are recovered with the third choice. However, fk(ρ̃;y) corresponds to 1+Ỹk(p̃,ρ̃) in [17], where p̃=y, and transformations (59)–(61) are defined with different coefficients in [17], using also a different definition of Kd. Here, we used the same form of the dimensionless equations as in [10,36], as it allowed us to adapt very easily the computational algorithms developed in [36] for the solution of the actual equations.

7 Calculation results

7.1 The method of solution

We solved the dimensionless equations of Sec. 6 in three dimensions (d = 3) as an example of the application of our general truncated equations within the BMW scheme, considering here the order s = 2. Moreover, we compared the results with those of the surprisingly similar equations in [10].

We used the method of semi-analytic approximations or functional truncations developed in [36]. According to this method, the dimensionless potential ũk(ρ̃) and the function fk(ρ̃;y) are represented as

ukρ̃uk0=1zμûkz,(71)
fkρ̃;y=f̄kz;y,(72)

where z=ρ̃/(ρ̃0+ρ̃) and μ = d/(d − 2 + η) (η being the fixed-point value of η(k)) with the following truncated expansions:

ûkz=m=1num,kzm,(73)
f̄kz;y=m=0nfm,kyzm.(74)

Here, ρ̃0 is an optimization parameter and μ is the exponent, which describes the power-law large-ρ̃ asymptotic of uk(ρ̃) at the fixed point. We used ρ̃0=0.4, as in most calculations in [36].

The coefficients um,k and fm,k(y) are calculated adapting the algorithm described in [36]. Namely, 12yf̄k(s;y)+y1f̄k(s;y1)+Yf̄k(s;Y) in Eq. 19 of [36], where now sz, is replaced by yf̄k(z;y) in the original BMW scheme and by yf̄k(z;y)+y1f̄k(z;y1) in the modified BMW scheme. Correspondingly, Eq. 62 of [36] becomes

Wi,ky,y1,Y=i+1wi+1,k+yfi+1,kyin the original BMW scheme,i+1wi+1,k+yfi+1,ky+y1fi+1,ky1in the modified BMW scheme.(75)

The integration of the RG flow equations (from t = 0 to t = −17) was performed by the fourth-order Runge–Kutta method, calculating fm,k(y) on a non-uniform grid of y values yn, where y0 = 0 and yn+1 = yn + (1 + ɛ)(ynyn−1) for n ≥ 1 and ynymax with large enough ymax to include the region q > Λ in the original variables. Typically, we used y1 = 0.02 and ɛ = 0.4, which corresponds to the “rough” grid considered in [36]. A similar “rough” grid with y1 = 0.002 and with restricted maximal step size 0.8 was used for the calculation of the integrals by the Simpson method, cutting the integration region at ymax = 30 and integrating over the angle θ with the step size π/5 (i.e., π/10 step size for subintervals).

Further details about the numerical procedures are provided in [36], noting that the “standard” grid has been mainly used there with twice smaller step sizes for y and θ. Here, we mainly use the “rough” grid, verifying in a subset of cases that the discrepancy with the results of the “standard” grid is practically negligible, as already pointed out in [36].

7.2 Estimation of the critical exponents η, ν, and ω

We extracted the critical exponents η, ν, and ω from the RG flow by a direct integration of the RG flow equations. In this case, the fixed point is reached by adjusting the initial condition iteratively, and the critical exponents are determined from the RG flow at and near the critical surface [36]. The critical exponent η describes the ∝ k−2+η divergence of the critical two-point correlation function, as well as the ∝ kη divergence of the renormalization constant Zk on the critical surface at k → 0. It is determined as the fixed-point value of the running exponent η(k). The critical exponent ν describes the ∝|τ|ν divergence of the correlation length at τ → 0, where τ is the deviation from the critical temperature. It describes also an infinitesimal deviation of the RG flow from the fixed point. It is extracted from a small ∝ k−1/ν deviation of this flow at small k values. The critical exponent ω describes corrections to scaling, as well as the ∝ kω distance of the RG flow from the fixed point on the critical surface at k → 0.

Practically, we determined the exponents yT = 1/ν and ω from the RG flow of the coupling coefficient u1,k in (73). We determined yT from the kyT scaling of ũ1,ku1,k, where ũ1,k is calculated slightly shifting (by 10–12) the initial value of u1,k at k = Λ from its critical value. The running exponent yT(k) was determined by using the ansatz ũ1,ku1,k=constkyT for k = k1 and k = k2, corresponding to t ±Δt with t = ln (k/Λ) and Δt ≈ 0.7. Thus, we used yT(k)=lnũ1,k2u1,k2/ũ1,k1u1,k1/[2Δt]. The running exponent ω(t) was extracted from the ansatz u1,k=u1*+constkω for three values of k, corresponding to t and t ±Δt with Δt ≈ 0.7. Hence, ω(k)=lnu1,k1u1,k/u1,ku1,k2/Δt and k1,2 = k exp (±Δt). The critical exponents ν and ω were determined as the asymptotic values of 1/yT(k) and ω(k) at k → 0, performing a tiny linear extrapolation of yT(k) and ω(k) over kω, based on the observation that these running exponents are almost linear in this scale.

For simpler RG flow equations, the critical exponents can be easily extracted from the linearized RG analysis in the vicinity of the fixed point. It is a standard method in the cases, where the RG flow is described by a finite number N of discrete parameters. It is true, e.g., for the LPA and the derivative expansion [11,14,15,18]. In this case, all the critical exponents, including the subleading correction-to-scaling exponents, are obtained as eigenvalues of the sensitivity matrix with dimensions N × N. Such a method cannot be easily applied to the equations with full momentum dependence in [10,17,36] and here, as one deals also with RG flow equations for continuous functions, in particular, for the functions fm,k(y) in (74). In [17], the critical exponents have been evaluated by a direct integration of the RG flow equations, like in our current study. A linearization around the fixed point, found by a fast iterative method without such integration, has been applied to equations with full momentum dependence in our earlier work [10]. However, it was only a toy example for a very simple approximation.

The critical exponents, evaluated here from the approximate RG flow equations with the dimensionless cut-off function (62), depend on the parameter α in (62). The exactly solved Wetterich equation would ensure the α-independence of these exponents; therefore, often such a value of α is assumed as optimal, at which the specific critical exponent shows a minimal variation with α. It is known as the principle of minimal sensitivity (PMS) [14]. In practice, the PMS values of η, ν, and ω appear to be the extremum points of the corresponding exponent vs. α plots. We found it meaningful to consider such plots depending on ln α rather than α. In this case, the plots appear to be more symmetric, and they are better approximated by spline curves. Moreover, the modulus of the local slope of such a plot is proportional to the magnitude of the variation when αα(1 + ɛ) at a small ɛ and, therefore, it serves as a good measure of the sensitivity.

The plots of the critical exponents η, ν, and ω vs. ln α, calculated at the truncation orders n = 13 and n′ = 10 in (73)(74), are shown in Figure 1. In this figure, the results of the (Secs. 5–6) approximate RG equations of the original BMW scheme, the modified BMW scheme, and the scheme of [10] considered here are shown. The PMS values correspond to the extremum points, indicated by the vertical dashed lines.

FIGURE 1
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FIGURE 1. Critical exponents η (A), ω (B), and ν (C) vs. ln α provided by the approximate RG flow equations (Sec. 6) of the original BMW scheme (squares), the modified BMW scheme (solid circles), and the scheme of [10] (empty circles), calculated at n = 13, n′ = 10 in (73)(74). The values obtained using the principle of minimal sensitivity correspond to the extremum points, indicated by the vertical dashed lines.

These PMS values are collected in Table 1. The values in the third row are taken from [36], where the indicated error bars have been estimated based on a detailed analysis of the convergence in (73)(74). We set the error bars in the first two rows in Table 1 based on a comparative analysis. We performed calculations at n = 10, n′ = 7 and found that the deviations in the critical exponents relative to those for n = 13, n′ = 10 strongly correlate in all three schemes considered and are comparable in magnitude with the corresponding error bars in row 3. For η and ν, these deviations in the BMW schemes are slightly (by 18% for ν and even less for η) larger than those in the scheme of [10]. For ω, they are at least by 38% smaller. In absence of a more detailed convergence test, we rounded up the expected error bars in rows 1–2.

TABLE 1
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TABLE 1. Values of the critical exponents η, ω, and ν, extracted from approximate RG flow equations (Sec. 6) of three schemes, using the principle of minimal sensitivity to find the optimal parameter α for each of the exponents, as shown in Figure 1.

The critical exponents obtained here for the original BMW scheme coincide with those reported in [17], i.e., η ≈ 0.039, ν ≈ 0.632, and ω ≈ 0.78. The estimates in Table 1 can be compared with those of the conformal field theory (CFT), i. e., η = 0.0362978(20), ν = 0.6299709 [38], and ω = 0.82951(61) [39], which are claimed to be very accurate. This comparison shows that the considered truncated RG equations give rather accurate values of ν, but the values of η are less accurate and somewhat overestimated.

Concerning ω, there are still some doubts about the acceptable value. Probably, the CFT value ωCFT = 0.82951 (61) is just the acceptable one. However, as discussed in [40], some numerical estimates, including the Monte Carlo renormalization group (MCRG) values ω ≈ 0.7 [42], ω = 0.75 (5) [42], the MCRG estimate from the reanalyzed data of [41] ω = 0.741 (21) [40], and the large mass expansion result ω ≈ 0.8002 [43] tend to give smaller ω values. Seeking for a compromise between these estimations, we set 0.76 as the lower bound for ω in our formal analysis. This choice is partly motivated by the fact that even smaller ω values would poorly fit in this analysis, where the refined estimates are expected to be at least slightly better than those of the LPA.

Thus, we consider ω = ωCFT as one option, allowing also a theoretical possibility that ω is smaller than ωCFT, but not smaller than 0.76. In this case, the actual RG estimates of η, ν, and ω in Table 1 are closer to the exact values than the corresponding PMS estimates of LPA, i. e., ηLPA = 0, νLPA = 0.650601 (10), and ωLPA = 0.654115 (30) [36] for the cut-off function (62). It can be seen from the values of the parameter

ζλ=λλexλλLPA,(76)

where λ = η, ν, ω is the actual RG estimate of the critical exponent, λex is its exact value, and λLPA is its LPA value. The parameters ζλ, calculated from the PMS values of λ and λLPA, are collected in Table 2. We evaluated ζω at ωex = ωCFT, ωex = 0.8, and ωex = 0.76 in (76) to see how this parameter changes if the exact ω value is 0.76 ≤ ωωCFT. It should be noted that ζλ > 1/2 would mean that the estimate of λ in Table 1 is worse than that of the LPA. It would be true for λ = ω in the scheme of [10] if ωex ≤ 0.757.

TABLE 2
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TABLE 2. Parameters ζλ with λ = η, ν, ω, calculated from the PMS values of the critical exponents (Table 1) of three truncation schemes. The last three rows contain ζω values for ωex = ωCFT (top), ωex = 0.8 (middle), and ωex = 0.76 (bottom) in (76).

We further used these parameters for a rough estimation of possible error bars for the subleading correction-to-scaling exponent ω2 in Sec. 7.3, assuming that |ζω2| does not essentially exceed the largest values of |ζλ| for λ = η, ν, ω.

7.3 Estimation of the critical exponent ω2

The developed techniques allow us to extract from the RG flow not only the leading correction-to-scaling exponent ω but also the subleading one ω2. To the best of our knowledge, it has not yet been obtained from the Wetterich equation beyond the LPA, where ω2 ≈ 3.18 has been reported in [15] for the actually considered scalar 3D model.

The RG flow is described by the state vector X depending on t, where X includes all the independent variables contained in the RG flow equations. In particular, considering our semi-analytic approximations, the components of X are the coefficients um,k in (73) and the functions fm,k(y) in (74). The RG flow equations have the form

tX=FX,t,(77)

where the explicit t dependence of F (X, t) shows up only in the upper cut-off and is irrelevant in vicinity of the fixed point X = X*. A standard method is to linearize X = X* + δX with respect to an infinitesimal deviation δX from the fixed point. It leads to the solution of the linearized RG, which has the form

δX=C1X1eωt+C2X2eω2t+Oeω3t(78)

on the critical surface at large −t values (t < 0), where ω is the leading correction-to-scaling exponent, ω2 > ω is the subleading correction-to-scaling exponent, ω3 > ω2 is the next exponent in this hierarchy of the eigenvalues, and Xi is the eigenvector corresponding to ωi (where ω1ω). For a unique representation, the eigenvectors are normalized appropriately. The constants Ci depend on the initial conditions.

Our basic idea is to find such initial conditions, at which C1 = 0. In this case, δXeω2t=kω2 holds in the linearized RG at t → −. Obviously, it holds also beyond the linearized RG since the non-linear corrections are those proportional to C1eωt2, C1eωt3, C1C2e(ω+ω2)t, etc., which are formally contained in O(δX)2. It means that all terms containing the exponent ω vanish at C1 = 0. It allows us to extract numerically the exponent ω2 from the RG flow at C1 = 0 just as we extracted ω at C1 ≠ 0.

A direct numerical extraction of ω2 from the RG flow at C1 ≠ 0 is difficult since δX contains a full set of correction terms in this case, including all ∝ k terms with integer n ≥ 1. The vanishing of all these ∝ k terms at C1 = 0 is a great advantage. We strictly verified numerically that these terms really vanish at C1 = 0. Namely, we have always obtained by our method such ω2 value, which is not just an integer multiple of ω, despite the fact that < ω2 holds for some n > 1.

We integrated the RG flow with a certain initial condition at k = k0, where k0 = Λ = 1, choosing fm,k0=δm,0, u3,k0=1, and um,k0=0 for m > 3. We set u2,k0=0.2, iteratively adjusting u1,k0 to the critical surface and determining the critical exponents η and ω, as described in Sec. 7.2. For the estimation of ω2, additional calculations were performed at different values of u2,k0 (adjusting u1,k0 for each of them to fit the critical surface) and finding such u2,k0 value u2,k0=u2+, at which the condition C1 = 0 is satisfied. At this condition, amplitude a of the leading scaling behavior u1,ku1*=akω at k → 0 (where u1* is the fixed-point value of u1,k) vanishes, and the scaling u1,ku1*kω2 is observed on the critical surface at k → 0, in agreement with our previous analysis.

Considering the running exponent ω(k) (calculated just as described in Sec. 7.2) for various u2,k0, we observe that ω(k) tends to a certain value ω2 > ω at a certain u2,k0=u2+. As an example, we show this in Figure 2 for the equations of the modified BMW scheme at α = 4.5 with n = 13 and n′ = 10 in (73)(74). We find from this set of curves that u2+0.6548703 and ω2 ≈ 1.962. The truncation error in (73)(74) was roughly estimated as the modulus of the difference (about 0.015) between the actual result and that one obtained at n = 10, n′ = 7. Taking into account also the uncertainty about 0.002 of the estimation in Figure 2 and rounding up the error bars, we have ω2 = 1.962 (20) in this example. Such results at selected values of α for all three schemes are collected in Table 3, whereas the plots of ω2 vs. α at n = 13, n′ = 10 are shown in Figure 3.

FIGURE 2
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FIGURE 2. Running exponent ω(k) in the modified BMW scheme at α = 4.5. From top to bottom u2,k0=0.654, 0.6547, 0.65485, 0.654867, 0.6548703, 0.654873, 0.6549, and 0.6554. The plot converges to ω2 ≈ 1.962 at u2,k0=u2+0.6548703.

TABLE 3
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TABLE 3. Subleading correction-to-scaling exponent ω2, obtained from approximate RG flow equations of three truncation schemes at the given values of parameter α in (62).

FIGURE 3
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FIGURE 3. ω2 vs. ln α plots, obtained from approximate RG flow equations of the modified BMW scheme (the upper curve) and the scheme of [10] (the lower curve). The interval α ∈ [1.99, 5.65] of the preferable α values is between the vertical dotted lines. Our final result ω2 = 2.02 (40), evaluated in the middle of the corresponding ln α interval at α = 3.353 is indicated by the dashed lines, showing the error bars by the horizontal dotted lines and the vertical arrows. The LPA value ω2LPA=3.14(7) at α = 3.353 is shown by the horizontal dot–dashed line for comparison.

Because of a poor scaling of ω(k) at u2,k0u2+, observed in the original BMW scheme at α ≤ 6.7, our ω2 results for this scheme are limited to α = 8 and α = 10, and the corresponding plot in Figure 3 is not shown. The maximal values of α (8.2 and 5.5), at which the results in the remaining two schemes were obtained, are limited by the problems of finding the solution with C1 = 0. In addition, the range of α values for the modified BMW scheme is restricted from below by α ≥ 2 because the ω(k) scaling appeared to be relatively poor at a smaller α value (α = 1.3) we considered.

The critical exponents η, ν, and ω are routinely estimated at the PMS values of α. The problem with ω2 is that no such α values can be identified in Figure 3. Moreover, an extrapolation of the plots in Figure 3 suggests that the extremum points, which could be identified with these PMS values, probably, are located at very large α values of about 20 or even >20. The choice of such α values as optimal ones seems to be doubtful since the overall accuracy of the solution is relatively low at α ∼ 20, i. e., η, ν, and ω deviate remarkably from the optimally estimated values.

The estimation can be performed at reasonable values of α, chosen according to some extra criteria. In particular, ω2 is determined from the RG flow on the critical subsurface, where C1 = 0 holds; therefore, it makes sense to consider such α values, which allow describing this flow as far as possible accurately. The critical exponents η and ω2 are relevant for this flow; therefore, we are looking for such α values, which are acceptable or preferable for the estimation of both these exponents simultaneously.

We focus mainly on the estimation of ω2 from the equations of the modified BMW scheme. This method is advantageous from the point of view that it appears to be much more accurate than the LPA if ω = ωCFT, as well as if ω has a significantly smaller value within [0.76, ωCFT]. It is evident from the coefficients ζλ in Table 2. We argue that preferable values of α for the estimation of ω2 from these equations are α[αoptη,5.65], where αoptη=1.99 is the optimal α value for the estimation of η. Indeed, both η and ω2 become more sensitive with respect to the variation of α if α is decreased below αoptη. Therefore, we choose α > 1.99. On the other hand, the deviation from the exact η value monotonously increases with α for α>αoptη and, at α = 5.65, becomes twice as large as at αoptη. Therefore, we consider α ∈ [1.99, 5.65] as preferable values of α, corresponding to the interval ln α ∈ [0.688, 1.732] between the vertical dotted lines in Figure 3. We choose ln α = 1.21 as an intuitively well-acceptable or nearly optimal ln α value in the middle of this interval. It gives ω2 = 2.017 (20), as shown in Figure 3 by the dashed lines. The error bars of ω2 = 2.017 (20) include only the uncertainty of this estimation at ln α = 1.21 or α = 3.353.

The estimation of the total error bars, including the systematic deviation from the exact value due to the closing approximation used in the modified BMW truncation scheme, is based on the assumption that, at appropriate α values (including α = 3.353), |ζω2| does not essentially exceed the largest value 0.252 of |ζλ| for λ = η, ν, ω in this scheme, see Table 2. We have set somewhat larger maximal value 0.3 for |ζω2| to increase the confidence level of our estimation. Thus, we evaluated the truncation error bars as 0.3ω2LPAω2, where ω2LPA is the LPA value of ω2 at α = 3.353 and ω2 = 2.017 (20) is our actual estimate at this α. We obtained ω2LPA=3.14(7) at α = 3.353 by our techniques, setting n′ = 0 in (74) and considering n ≤ 13 in (73). This LPA value is close to ω2LPA3.18 reported in [15]. Taking into account all error estimates in our calculations, our final result is

ω2=2.0240(79)

for the scalar model in three dimensions, which belongs to the 3D Ising universality class. Although the error bars in (79) are not rigorous, no much larger discrepancy with the exact value is expected according to the arguments provided. These arguments basically rely on the assumption that the convergence of ω2 values, estimated at the truncation orders s = 0, 2, 3, 4, etc., in the modified BMW scheme, would not be essentially slower than the convergence for all other exponents (η, ν, and ω) considered here. Since the actual results include only the cases s = 0 and s = 2, no strict validation of this assumption is possible at the moment; therefore, the error bars in (79) are preliminary. From this point of view, one could allow even larger error bars, but the current information is insufficient to state how much larger. It can be clarified by extended calculations at higher orders.

The error bars of this estimation and the LPA value are shown in Figure 3 for an analysis and comparison. The results extracted from the equations of [10] support (79) since the corresponding lower curve in Figure 3 well fits within these error bars. This estimate agrees also with the RG value ω2 = 1.67 (11) obtained earlier in [37] from the approximated Polchinski RG equation within the derivative expansion at the O2 order. The relatively small (as compared to ours) error bars stated for this value presumably reflect only the uncertainty of the estimation from this approximate equation.

8 Summary and outlook

In this section, we give a brief summary of the obtained results, as well as discuss some possible further applications and developments.

In the current paper, we reported our new developments in the BMW truncation scheme for the Wetterich non-perturbative RG equation. We derived explicit RG flow equations for the scalar model at the arbitrary order of truncation, proposing also new closing approximations for the hierarchy of equations for the n-point functions in the BMW scheme (Sec. 4). A surprising similarity between the original and the modified equations of the BMW scheme at s = 2 order of truncation and those recently reported in [10] was shown (Secs. 5–6). As an example, calculations of the critical exponents for the 3D scalar model were performed, solving these equations by the method of semi-analytic approximations recently proposed in [36] (Sec. 7).

Particularly, the subleading correction-to-scaling exponent ω2 has been evaluated from the Wetterich equation beyond the LPA. Our estimate ω2 = 2.02 (40) is significantly smaller than the LPA value 3.18 reported in [15] and compares well with the value ω2 = 1.67 (11), obtained in [37] from the Polchinski equation at the O2 order of DE. The error bars of our estimate ω2 = 2.02 (40) are relatively large because they include the expected truncation error due to the closing approximation in the BMW scheme.

The calculations of ω2 demonstrate the usefulness of our new developments. In particular, just the modified equations of the BMW scheme and those derived in [10] appeared to be practically most useful for these calculations, allowing obtaining the results at reasonable values of the optimization parameter α.

The estimation of the critical exponent ω2 is crucial for testing the consistency between the RG exponents and those of the CFT. While the RG critical exponents η, ν, and ω appear to be reasonably close to the corresponding CFT values (see Sec. 7.2), there is clearly a problem with ω2. As already pointed out in Sec. 1, the known estimation in [37] gives a much smaller ω2 (i. e., ω2 = 1.67 (11)) than the CFT value 3.8956 (43) [39]. Our current estimation ω2 = 2.02 (40) allows for significantly larger than 1.67 values; however, these are still very small to speak about a consistency with CFT. In fact, the current estimations urge us to think that the RG exponent ω2, probably, is unrelated to the conformal symmetry since the RG values appear to be incompatibly smaller than 3.8956 (43).

The proposed scheme has the potential for various applications in calculations at higher than s = 2 orders. In particular, it would help in a further clarification of the question about the relation between the RG exponents and the CFT exponents. Development of improved solution techniques would be quite important for such calculations. Following [44,45], an interesting option is to use the expansion in Chebyshev polynomials for semi-analytic approximations. It could be an advantageous method owing to the guaranteed fast convergence properties of such expansions [45]. These can be used as an alternative to the expansions in powers of z in (73)(74). One can also think about appropriate semi-analytic approximations for the momentum dependence of the n-point functions to make the calculations at higher than s = 2 orders more feasible.

Apart from very extensive and systematic applications of the non-perturbative RG approach to equilibrium statistical physics, it has also been applied to the out-of-equilibrium systems and critical dynamics [3234]. The employed truncation schemes include the LPA and its refined modification [34]. There is still room for potential applications of other truncation schemes, including the currently introduced modified BMW scheme, which could be adjusted to this problem. It would be a quite interesting application, eventually, allowing obtaining refined RG estimates for the dynamical exponent z. Indeed, the actual estimates of this exponent are not very accurate, and there is a continued discussion of z values obtained from Monte Carlo simulations, experiments, and RG equations [34, 46].

Data availability statement

The raw data supporting the conclusion of this article will be made available by the authors, without undue reservation.

Author contributions

All authors listed made a substantial, direct, and intellectual contribution to the work and approved it for publication.

Acknowledgments

The authors acknowledge the Latvian Grid Infrastructure and High Performance Computing Centre of Riga Technical University for providing resources. JK acknowledges the support from the Science Support Fund of Riga Technical University. RM acknowledges the support from the NSERC and CRC programs.

Conflict of interest

The authors declare that the research was conducted in the absence of any commercial or financial relationships that could be construed as a potential conflict of interest.

Publisher’s note

All claims expressed in this article are solely those of the authors and do not necessarily represent those of their affiliated organizations, or those of the publisher, the editors, and the reviewers. Any product that may be evaluated in this article, or claim that may be made by its manufacturer, is not guaranteed or endorsed by the publisher.

Supplementary material

The Supplementary Material for this article can be found online at: https://www.frontiersin.org/articles/10.3389/fphy.2023.1182056/full#supplementary-material

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Keywords: functional renormalization, Wetterich equation, truncation schemes, exact renormalization group equations, non-perturbative approaches, quantum and statistical field theories, strongly interacting systems

Citation: Kaupužs J and Melnik RVN (2024) Original and modified non-perturbative renormalization group equations of the BMW scheme at the arbitrary order of truncation. Front. Phys. 11:1182056. doi: 10.3389/fphy.2023.1182056

Received: 08 March 2023; Accepted: 01 December 2023;
Published: 15 January 2024.

Edited by:

Manuel Asorey, University of Zaragoza, Spain

Reviewed by:

Frank Simon Saueressig, Radboud University, Netherlands
Gerd Roepke, University of Rostock, Germany

Copyright © 2024 Kaupužs and Melnik. This is an open-access article distributed under the terms of the Creative Commons Attribution License (CC BY). The use, distribution or reproduction in other forums is permitted, provided the original author(s) and the copyright owner(s) are credited and that the original publication in this journal is cited, in accordance with accepted academic practice. No use, distribution or reproduction is permitted which does not comply with these terms.

*Correspondence: J. Kaupužs, kaupuzs@latnet.lv

Disclaimer: All claims expressed in this article are solely those of the authors and do not necessarily represent those of their affiliated organizations, or those of the publisher, the editors and the reviewers. Any product that may be evaluated in this article or claim that may be made by its manufacturer is not guaranteed or endorsed by the publisher.