# Bell Polynomials Approach Applied to (2 + 1)-Dimensional Variable-Coefficient Caudrey-Dodd-Gibbon-Kotera-Sawada Equation

Authors: Wen-guang Cheng; Biao Li; Yong Chen
Journal: Abstract and Applied Analysis
 (2014)

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## Abstract

The bilinear form, bilinear Bäcklund transformation, and Lax pair of a (2 + 1)-dimensional variable-coefficient Caudrey-Dodd-Gibbon-Kotera-Sawada equation are derived through Bell polynomials. The integrable constraint conditions on variable coefficients can be naturally obtained in the procedure of applying the Bell polynomials approach. Moreover, theN-soliton solutions of the equation are constructed with the help of the Hirota bilinear method. Finally, the infinite conservation laws of this equation are obtained by decoupling binary Bell polynomials. All conserved densities and fluxes are illustrated with explicit recursion formulae.


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## Body

## 1. Introduction

It is well known that investigation of integrable properties of nonlinear evolution equations (NEEs) can be considered as a pretest and the first step of its exact solvability. The integrability features of soliton equations can be characterized by Hirota bilinear form, Lax pair, infinite symmetries, infinite conservation laws, Painlevé test, Hamiltonian structure, Bäcklund transformation (BT), and so on. The bilinear form of a soliton equation can not only be used to produce many of the known families of multisoliton solutions, but also be employed to derive the bilinear BT, Lax pair, and infinite sets of conserved quantities [1–6]. However, it relies on a particular skill and tedious calculation. In the early 1930s, the classical Bell polynomials were introduced by Bell which are specified by a generating function and exhibiting some important properties [7]. Recently, Lambert and coworkers have proposed a relatively convenient procedure based on Bell polynomials which enables us to obtain bilinear forms, bilinear BTs, Lax pairs, and Darboux covariant Lax pairs for NEEs [8–11]. It is shown that Bell polynomials play an important role in the characterization of bilinearizable equations and a deep relation between the integrability of an NEE and the Bell polynomials. Furthermore, Fan [12], Fan and Chow [13], and Wang and Chen [14, 15] developed the approach to construct infinite conservation laws by decoupling binary-Bell-polynomial-type BT into a Riccati type equation and a divergence type equation. Afterwards, Fan [16] and Fan and Hon [17] extended this method to supersymmetric equations. On the basis of their work, we apply the bell polynomials approach to the high-dimensional variable-coefficient NEEs.Many physical and mechanical situations are governed by variable-coefficient NEEs, which might be more realistic than the constant coefficient ones in modeling a variety of complex nonlinear phenomena in physical and engineering fields [18–20].The (2 + 1)-dimensional analogue of the Caudrey-Dodd-Gibbon-Kotera-Sawada (CDGKS) equation is in the form of(1)36ut=-u5x-15(uu2x)x-45u2ux+5u2x,y+15uuy+15ux∂x-1uy+5∂x-1u2y,with∂x-1=∫·dx. Equation (1) is first proposed by Konopelchenko and Dubrovsky [21] and then considered by many authors in various aspects such as its quasiperiodic solutions [22], algebraic-geometric solution [23], N-soliton solutions [24], nonlocal symmetry [25], and symmetry reductions [26]. Based on (1), we will consider a (2 + 1)-dimensional variable-coefficient CDGKS equation as
(2)ut+a1u5x+a2uxu2x+a3uu3x+a4u2ux+a5u2x,y+a6∂x-1u2y+a7ux∂x-1uy+a8uuy+a9u=0,whereai=ai(t), i=1,…,9, are analytic functions with respect to t. The aim of this paper is applying the Bell polynomials approach to systematically investigate the integrability of (2), which includes bilinear form, bilinear BT, Lax pair, and infinite conservation laws.The layout of this paper is as follows. Basic concepts and identities about Bell polynomials will be briefly introduced in Section2. In Section 3, by virtue of Bell polynomials and the Hirota bilinear method, the bilinear form and N-soliton solutions of (2) are obtained. In Sections 4 and 5, with the aid of Bell polynomials, the bilinear BT, Lax pair, and infinite conservation laws of (2) are systematically presented, respectively. Section 6 will be our conclusions.


## 2. Bell Polynomials

The Bell polynomials [7, 9, 10] used here are defined as
(3)Ynx(f)=Yn({frx(1≤r≤n)})=e-f∂xnef,Y0x≡1,wheref(x) is a C∞ function and frx=∂xrf; according to formula (3), the first three are
(4)Yx(f)=fx,Y2x(f)=f2x+fx2,Y3x(f)=f3x+3fxf2x+fx3.Based on one-dimensional Bell polynomials, the multidimensional Bell polynomials are expressed as(5)Yn1x1,…,nlxl(f)=Yn1,…,nl({fr1x1,…,rlxl(1≤ri≤ni,0≤i≤l)})=e-f∂x1n1⋯∂xlnlef,withf=f(x1,…,xl) being a C∞ function and fr1x1,…,rlxl=∂x1r1⋯∂xlrlf; the associated two-dimensional Bell polynomials can be written as
(6)Ymx,nt(f)=Ym,n({frx,st(1≤r≤m,1≤s≤n)})=e-f∂xm∂tnef.The most important multidimensional binary Bell polynomials, namely,Y-polynomials, can be defined as
(7)Yn1x1,…,nlxl(v,w)=Yn1x1,…,nlxl(f)=Yn1,…,nl({fr1x1,…,rlxl})for(8)fr1x1,…,rlxl={vr1x1,…,rlxl∑i=0l‍riisoddwr1x1,…,rlxl∑i=0l‍riisevenwith the first few lowest order binary Bell polynomials being(9)Yx(v)=vx,Y2x(v,w)=w2x+vx2,Yx,t(v,w)=wx,t+vxvt,Y2x,t(v,w)=v2x,t+w2xvt+2wxyvx+vx2vy,….TheY-polynomials can be linked to the standard Hirota expressions through the identity [10]
(10)Yn1x1,…,nlxl(v=ln⁡(FG),w=ln⁡(FG))=(FG)-1Dx1n1⋯DxlnlF·G,in which∑i=1lni≥1 and the operators Dx1n1⋯Dxlnl are classical Hirota bilinear operators defined by [1]
(11)Dx1n1⋯DxlnlF·G=(∂x1-∂x1′)n1⋯(∂xl-∂xl′)nl×F(x1,…,xl)G(x1′,…,xl′)|x1′=x1,…,xl′=xl.Introducing a new fieldq=w-v, in the particular case F=G one has
(12)G-2Dx1n1⋯DxlnlG·G=Yn1x1,…,nlxl(0,q=w-v)={0∑i=0l‍niisodd,Pn1x1,…,nlxl(q)∑i=0l‍niiseven,in which the even-orderY-polynomials is called P-polynomials; that is,
(13)Pn1x1,…,nlxl(q)=Yn1x1,…,nlxl(0,q=w-v),with(14)P2x(q)=q2x,Px,t(q)=qx,t,P4x(q)=q4x+3q2x2,P6x(q)=q6x+15q2xq4x+15q2x3,….Moreover, the binary Bell polynomialsYn1x1,…,nlxl(v,w) can be written as the combination of P-polynomials and Y-polynomials:
(15)(FG)-1Dx1n1⋯DxlnlF·G=Yn1x1,…,nlxl(v,w)|v=ln⁡(F/G),w=ln⁡(FG)=Yn1x1,…,nlxl(v,v+q)|v=ln⁡⁡(F/G),q=2ln⁡G=∑p1=0n1‍⋯∑pl=0nl‍(n1p1)⋯(nlpl)Pn1x1,…,nlxl(q)sssssssssss×Y(n1-r1)x1,…,(nl-rl)xl(v).Under the Hopf-Cole transformationv=ln⁡ψ, the Y-polynomials can be linearized into the form
(16)Yn1x1,…,nlxl(v)|v=ln⁡ψ=ψn1x1,…,nlxlψ,which provides a straightforward way for the related Lax systems of NEEs.


## 3. Bilinear Form andN-Soliton Solutions for (2)

Firstly, introduce a dimensionless potential fieldq by setting
(17)u=cq2x,withc=c(t) to be determined. Substituting (17) into (2), integration with respect to x yields the following potential version of (2):
(18)(ctc+a9)qx+qx,t-16c(a7-a8)∂x-1∂y(q4x+3q2x2)+a1q6x+12c(a2-a3)q3x2+ca3q2xq4x+13c2a4q2x3+[a5+16c(a7-a8)]q3x,y+a6q2y+ca7q2xqx,y=0;on account of the dimension ofu (dim⁡u=-2), we find that setting c=c0e-∫a9dt, where c0 is an arbitrary constant. In order to write (18) in local bilinear form, here are two cases which are considered to eliminate the effect of the integration ∂x-1. The bilinear form and N-soliton solutions for each case will be discussed by selecting appropriate constraints on variable coefficients ai, i=1,…,9.


### 3.1. Case 1

Leta7=a8; (18) becomes
(19)qx,t+a1q6x+12c(a2-a3)q3x2+ca3q2xq4x+13c2a4q2x3+a5q3x,y+a6q2y+ca7q2xqx,y=0.This equation can be viewed as a homogeneousP-condition [8] of weight 6 (the weight of each term being defined as minus its dimension, a weight 3 to y). That means (19) can be written as a linear combination of P-polynomials of weight 6:
(20)Px,t(q)+a1P6x(q)+a5P3x,y(q)+a6P2y(q)=0;under the following constraint condition:(21)ca3-15a1=0,ca7-3a5=0,12c(a2-a3)=0,13c2a4-15a1=0,namely,(22)a2=a3=15a1c0e∫‍a9dt,a4=45a1c02e2∫‍a9dt,a7=a8=3a5c0e∫‍a9dt.According to the property (12), via the following transformation:
(23)q=2ln⁡G⟺u=cq2x=2c0e-∫‍a9dt(ln⁡G)2x,P-polynomials expression (20) produces the bilinear form of (2) as follows:
(24)(DxDt+a1Dx6+a5Dx3Dy+a6Dy2)G·G=0.Starting from this bilinear equation, the one-soliton solution of (2) can be easily obtained by regular perturbation method
(25)u=2c0e-∫‍a9dt[ln⁡(1+eη1)]2x,with(26)η1=k1x+l1y+ω1(t)+ξ1,ω1(t)=-∫‍k16a1+k13l1a5+l12a6k1dt.However, the multisoliton solutions cannot be derived by means of bilinear equation (24). For the sake of obtaining multisoliton solutions of (2), we take
(27)a5=5c1a1,a6=-5c12a1,wherec1 is an arbitrary constant; the bilinear equation can be expressed as
(28)(DxDt+a1Dx6+5c1a1Dx3Dy-5c12a1Dy2)G·G=0,with the conditions (22) and (27); that is,
(29)a2=a3=15a1c0e∫‍a9dt,a4=45a1c02e2∫‍a9dt,a5=5c1a1,a6=-5c12a1,a7=a8=15c1a1c0e∫‍a9dt.Based on the bilinear equation (28), the N-soliton solutions for (2) can be constructed as
(30)u=2c0e-∫‍a9dt[ln⁡(∑μ=0,1‍e∑j=1Nμjηj+∑1≤i<jNμiμjAij)]2x,where(31)ηj=kjx+ljy+ωj(t)+ξj,ωj(t)=-kj6+5c1kj3lj-5c12lj2kj∫‍a1dt,eAij={(kilj-kjli)2(ki-kj)[c1kikj2li(2ki-kj)+c1ki2kjlj(ki-2kj)ssssssssssssssss+ki2kj2(ki2-kikj+kj2)(ki-kj)]sssss+c12(kilj-kjli)2}×{(kilj-kjli)2(ki+kj)[c1kikj2li(2ki+kj)ssssssssssssssssssss+c1ki2kjlj(ki+2kj)ssssssssssssssssssss+ki2kj2(ki2+kikj+kj2)ssssssssssssssssssss×(ki+kj)]+c12(kilj-kjli)2}-1,withkj, lj, and ξj(j=1,2,…,N) being arbitrary constants; ∑μ=0,1 indicates a summation over all possible combinations of μj=0,1(j=1,2,…,N). For N=1, the one-soliton solution for (2) can be written as follows:
(32)u=12c0k12e-∫‍a9dt×sech2[12(k1x+l1y-k16+5c1k13l1-5c12l12k1sssssssfff×∫a1dt+ξ112k16+5c1k13l1-5c12l12k1)12].ForN=2, we can obtain the two-soliton solution for (2) as
(33)u=2c0e-∫‍a9dt[ln⁡(1+eη1+eη2+eη1+η2+A12)]2x.Based on solutions (32) and (33), we present some figures to describe the propagations and collisions of the solitary waves. Figure 1 shows the propagation of one-soliton solution via solution (32) when t=-2, t=-1, and t=2, which maintains its shape except for the phase shift, and the propagation direction can be changed. Figures 2 and 3 illustrate the oblique collision between the two solitons, which keep their original shapes invariant except for phase shifts as mentioned above. It is obvious that the large-amplitude soliton moves faster than the small one. Different from Figure 2, Figure 3 displays that both solitons change their directions during the collision.One-soliton solution via solution (32) with a9=0.01, k1=1, l1=2, c0=1, c1=1, a1=sin(t), and ξ1=0. (a) t=-2; (b) t=-1; (c) t=2.
(a)
(b)
(c)Two-soliton solution via solution (33) with a9=0.01, k1=1, k2=2, l1=2, l2=8, c0=1, c1=0.02, a1=0.2, and ξ1=ξ2=0. (a) t=-2; (b) t=0; (c) t=2.
(a)
(b)
(c)Two-soliton solution via solution (33) with a9=0.01, k1=1, k2=2, l1=2, l2=7, c0=1, c1=0.02, a1=t, and ξ1=ξ2=0. (a) t=-0.8; (b) t=0; (c) t=0.8.
(a)
(b)
(c)


### 3.2. Case 2

As another case, we introduce an auxiliary variables and a subsidiary condition
(34)q4x+3q2x2+qx,s=0,in virtue of which, similarly, (18) can be written as a linear combination of P-polynomials of weight 6 (a weight 3 to s):
(35)Px,t(q)+βP6x(q)+γP3x,y(q)+a6P2y(q)+16c(a7-a8)Py,s(q)+δP3x,s(q)+αPs,s(q)=0,with the following constraint condition:(36)ca7-3γ=0,a5-γ+16c(a7-a8)=0,ca3-15β+9δ-12α=0,a1-β+δ-α=0,13c2a4-15β+9δ-12α=0,12c(a2-a3)+6δ-3α=0.Solving for (36) yields
(37)γ=13c0e-∫‍a9dta7,β=-32a1+16c0e-∫‍a9dta3-12α,δ=-52a1+16c0e-∫‍a9dta3+12α,a2=-a3+30a1c0e∫‍a9dt,a4=3a3c0e∫‍a9dt,a5=16c0e-∫‍a9dt(a7+a8).Thus, theP-polynomials expression of (2) and (34) reads
(38)P4x(q)+Px,s(q)=0,Px,t(q)+(-32a1+16c0e-∫‍a9dta3-12α)P6x(q)+13c0e-∫‍a9dta7P3x,y(q)+a6P2y(q)+16c0e-∫‍a9dt(a7-a8)Py,s(q)+(-52a1+16c0e-∫‍a9dta3+12α)P3x,s(q)+αPs,s(q)=0,in whichα=α(t) is an arbitrary function.System (38) produces the bilinear form of (2) as follows:
(39)(Dx4+DxDs)G·G=0,[DxDt+(-32a1+16c0e-∫‍a9dta3-12α)Dx6+13c0e-∫‍a9dta7Dx3Dy+a6Dy2+16c0e-∫‍a9dt(a7-a8)DyDs+(-52a1+16c0e-∫‍a9dta3+12α)×Dx3Ds+αDs232]G·G=0,by property (12) and transformation (23). From the bilinear equation (39), we can only get the one-soliton solution which is the same as the above formulae (25) and (26). Therefore, (2) under the constraint conditions (37) is not integrable since its multisoliton solutions cannot be obtained.


## 3.1. Case 1

Leta7=a8; (18) becomes
(19)qx,t+a1q6x+12c(a2-a3)q3x2+ca3q2xq4x+13c2a4q2x3+a5q3x,y+a6q2y+ca7q2xqx,y=0.This equation can be viewed as a homogeneousP-condition [8] of weight 6 (the weight of each term being defined as minus its dimension, a weight 3 to y). That means (19) can be written as a linear combination of P-polynomials of weight 6:
(20)Px,t(q)+a1P6x(q)+a5P3x,y(q)+a6P2y(q)=0;under the following constraint condition:(21)ca3-15a1=0,ca7-3a5=0,12c(a2-a3)=0,13c2a4-15a1=0,namely,(22)a2=a3=15a1c0e∫‍a9dt,a4=45a1c02e2∫‍a9dt,a7=a8=3a5c0e∫‍a9dt.According to the property (12), via the following transformation:
(23)q=2ln⁡G⟺u=cq2x=2c0e-∫‍a9dt(ln⁡G)2x,P-polynomials expression (20) produces the bilinear form of (2) as follows:
(24)(DxDt+a1Dx6+a5Dx3Dy+a6Dy2)G·G=0.Starting from this bilinear equation, the one-soliton solution of (2) can be easily obtained by regular perturbation method
(25)u=2c0e-∫‍a9dt[ln⁡(1+eη1)]2x,with(26)η1=k1x+l1y+ω1(t)+ξ1,ω1(t)=-∫‍k16a1+k13l1a5+l12a6k1dt.However, the multisoliton solutions cannot be derived by means of bilinear equation (24). For the sake of obtaining multisoliton solutions of (2), we take
(27)a5=5c1a1,a6=-5c12a1,wherec1 is an arbitrary constant; the bilinear equation can be expressed as
(28)(DxDt+a1Dx6+5c1a1Dx3Dy-5c12a1Dy2)G·G=0,with the conditions (22) and (27); that is,
(29)a2=a3=15a1c0e∫‍a9dt,a4=45a1c02e2∫‍a9dt,a5=5c1a1,a6=-5c12a1,a7=a8=15c1a1c0e∫‍a9dt.Based on the bilinear equation (28), the N-soliton solutions for (2) can be constructed as
(30)u=2c0e-∫‍a9dt[ln⁡(∑μ=0,1‍e∑j=1Nμjηj+∑1≤i<jNμiμjAij)]2x,where(31)ηj=kjx+ljy+ωj(t)+ξj,ωj(t)=-kj6+5c1kj3lj-5c12lj2kj∫‍a1dt,eAij={(kilj-kjli)2(ki-kj)[c1kikj2li(2ki-kj)+c1ki2kjlj(ki-2kj)ssssssssssssssss+ki2kj2(ki2-kikj+kj2)(ki-kj)]sssss+c12(kilj-kjli)2}×{(kilj-kjli)2(ki+kj)[c1kikj2li(2ki+kj)ssssssssssssssssssss+c1ki2kjlj(ki+2kj)ssssssssssssssssssss+ki2kj2(ki2+kikj+kj2)ssssssssssssssssssss×(ki+kj)]+c12(kilj-kjli)2}-1,withkj, lj, and ξj(j=1,2,…,N) being arbitrary constants; ∑μ=0,1 indicates a summation over all possible combinations of μj=0,1(j=1,2,…,N). For N=1, the one-soliton solution for (2) can be written as follows:
(32)u=12c0k12e-∫‍a9dt×sech2[12(k1x+l1y-k16+5c1k13l1-5c12l12k1sssssssfff×∫a1dt+ξ112k16+5c1k13l1-5c12l12k1)12].ForN=2, we can obtain the two-soliton solution for (2) as
(33)u=2c0e-∫‍a9dt[ln⁡(1+eη1+eη2+eη1+η2+A12)]2x.Based on solutions (32) and (33), we present some figures to describe the propagations and collisions of the solitary waves. Figure 1 shows the propagation of one-soliton solution via solution (32) when t=-2, t=-1, and t=2, which maintains its shape except for the phase shift, and the propagation direction can be changed. Figures 2 and 3 illustrate the oblique collision between the two solitons, which keep their original shapes invariant except for phase shifts as mentioned above. It is obvious that the large-amplitude soliton moves faster than the small one. Different from Figure 2, Figure 3 displays that both solitons change their directions during the collision.One-soliton solution via solution (32) with a9=0.01, k1=1, l1=2, c0=1, c1=1, a1=sin(t), and ξ1=0. (a) t=-2; (b) t=-1; (c) t=2.
(a)
(b)
(c)Two-soliton solution via solution (33) with a9=0.01, k1=1, k2=2, l1=2, l2=8, c0=1, c1=0.02, a1=0.2, and ξ1=ξ2=0. (a) t=-2; (b) t=0; (c) t=2.
(a)
(b)
(c)Two-soliton solution via solution (33) with a9=0.01, k1=1, k2=2, l1=2, l2=7, c0=1, c1=0.02, a1=t, and ξ1=ξ2=0. (a) t=-0.8; (b) t=0; (c) t=0.8.
(a)
(b)
(c)


## 3.2. Case 2

As another case, we introduce an auxiliary variables and a subsidiary condition
(34)q4x+3q2x2+qx,s=0,in virtue of which, similarly, (18) can be written as a linear combination of P-polynomials of weight 6 (a weight 3 to s):
(35)Px,t(q)+βP6x(q)+γP3x,y(q)+a6P2y(q)+16c(a7-a8)Py,s(q)+δP3x,s(q)+αPs,s(q)=0,with the following constraint condition:(36)ca7-3γ=0,a5-γ+16c(a7-a8)=0,ca3-15β+9δ-12α=0,a1-β+δ-α=0,13c2a4-15β+9δ-12α=0,12c(a2-a3)+6δ-3α=0.Solving for (36) yields
(37)γ=13c0e-∫‍a9dta7,β=-32a1+16c0e-∫‍a9dta3-12α,δ=-52a1+16c0e-∫‍a9dta3+12α,a2=-a3+30a1c0e∫‍a9dt,a4=3a3c0e∫‍a9dt,a5=16c0e-∫‍a9dt(a7+a8).Thus, theP-polynomials expression of (2) and (34) reads
(38)P4x(q)+Px,s(q)=0,Px,t(q)+(-32a1+16c0e-∫‍a9dta3-12α)P6x(q)+13c0e-∫‍a9dta7P3x,y(q)+a6P2y(q)+16c0e-∫‍a9dt(a7-a8)Py,s(q)+(-52a1+16c0e-∫‍a9dta3+12α)P3x,s(q)+αPs,s(q)=0,in whichα=α(t) is an arbitrary function.System (38) produces the bilinear form of (2) as follows:
(39)(Dx4+DxDs)G·G=0,[DxDt+(-32a1+16c0e-∫‍a9dta3-12α)Dx6+13c0e-∫‍a9dta7Dx3Dy+a6Dy2+16c0e-∫‍a9dt(a7-a8)DyDs+(-52a1+16c0e-∫‍a9dta3+12α)×Dx3Ds+αDs232]G·G=0,by property (12) and transformation (23). From the bilinear equation (39), we can only get the one-soliton solution which is the same as the above formulae (25) and (26). Therefore, (2) under the constraint conditions (37) is not integrable since its multisoliton solutions cannot be obtained.


## 4. Bilinear BT and Lax Pair for (2)

In order to search for the bilinear BT and Lax pair of (2), under the integrable constraint condition (29) in case 1, we have
(40)E(q)=qx,t+a1(q6x+15q2xq4x+15q2x3)+5c1a1(q3x,y+3q2xqx,y)-5c12a1q2y=0.Let(41)q=2ln⁡G,q′=2ln⁡Fbe two solutions of (40), respectively. On introducing two new variables
(42)v=q′-q2=ln⁡(FG),w=q′+q2=ln⁡(FG),one has the corresponding two-field condition(43)E(q′)-E(q)=E(w+v)-E(w-v)=2[vx,t+15a1v2x3sss+(15a1w4x+45a1w2x2+15c1a1wxy)v2xsss-5c12a1v2y+a1v6x+15a1w2xv4xsss+5c1a1v3x,y+15c1a1w2xvx,yv2x3]=2∂x[Yt(v)+a1Y5x(v,w)+5c1a1Y2x,y(v,w)]+2R(v,w)=0,with(44)R(v,w)=-5a1(vx4v2x+2w3xvx3+6w2xvx2v2x+c1vx,yvx2+2v4xvx2+2c1v2xvxvy+2c1w2xyvx+4v3xvxv2x+6w2xvxw3x+w5xvx+c1w3xvy-3v2x3-6w2x2v2x-c1v2xwxy-2w4xv2x-2c1w2xvxy+c12v2y-v4xw2x+2v3xw3x).The simplest possible choice is a homogeneousY-constraint[8] of weight 2; it can only be of form
(45)Y2x(v,w)+aYy(v)=λ.It is easy to find that eliminatingw2x (and its derivatives) by means of form (45) does not enable one to express the remainder R(v,w) as the x-derivative of a linear combination of Y-polynomials. However, a homogeneous Y-constraint of weight 3
(46)Y3x(v,w)+c1Yy(v)=λ,λ=arbitraryparameterofweight3,can be used to expressR(v,w) as follows:
(47)R(v,w)=-52a1∂x[Y5x(v,w)-c1Y2x,y(v,w)sssssss+3λY2x(v,w)c1Y2x,yY5x(v,w)].Thus, the two-field condition (43) becomes
(48)∂x[Yt(v)-32a1Y5x(v,w)+152c1a1Y2x,y(v,w)s-152a1λY2x(v,w)]=0(weight6),where we prefer the equation in the conserved form, which is useful to construct conservation laws later. It is seen that the two-field condition (43) can be decoupled into a pair of parameter-dependent Y-constraints (of weight 3 and weight 5):
(49)Y3x(v,w)+c1Yy(v)-λ=0,Yt(v)-32a1Y5x(v,w)+152c1a1Y2x,y(v,w)-152a1λY2x(v,w)=0.In view of (10), the bilinear BT for (2) is obtained:
(50)(Dx3+c1Dy-λ)F·G=0,(Dt-32a1Dx5+152c1a1Dx2Dy-152a1λDx2)F·G=0.By application of formulae (15) and (16), the system (50) is linearized to be the Lax pair of (2) as
(51)ψ3x+3q2xψx+c1ψy=λψ,ψt-9a1ψ5x-45a1q2xψ3x-45q3xψ2x-(30a1q4x+45a1q2x2-15c1a1qx,y)ψx=0.Starting from this Lax pair witha1=-1, a9=0, c0=3, and c1=1, the Darboux transformation and nonlocal symmetry of the equation can be established [25]. Checking that the compatibility condition of system (51) is just the potential of (40).


## 5. Infinite Conservation Laws for (2)

In what follows, we present the infinite conservation laws by recursion formulae for (2). The conservation laws actually have been hinted in the binary-Bell-polynomial-type BT (46) and (48), which can be rewritten in the conserved form
(52)v3x+3vxw2x+vx3+c1vy=λ,∂t(vx)+∂x[-32a1(vx5v5x+5w4xvx+10v3xw2xssssssssssssssssssssss+10v3xvx2+15w2x2vxssssssssssssssssssssss+10w2xvx3+vx5)ssssssssssssss-152a1λ(w2x+vx2)ssssssssssssss+152c1a1(w2xvy+2wx,yvx+vx2vy)-32]+∂y(152c1a1v3x)=0,by using the relation(53)∂t(vx)=∂x(vt)=vx,t,∂y(vx)=∂x(vy)=vx,y.By introducing a new potential function(54)η=qx′-qx2,in this way, there are(55)vx=η,wx=qx+η.Substituting (55) into system (52), we obtain
(56)η2x+3η(q2x+ηx)+η3+c1∂x-1ηy=λ=ε3,(57)ηt+∂x[-32a1(η5η4x+5q4xη+5η3xη+10q2xη2xssssssssssssss+10ηxη2x+10η2η2x+15q2x2ηssssssssssssss+30q2xηxη+15ηx2η+10q2xη3ssssssssssssss+10ηxη3+η5)ssssss-152a1ε3(q2x+ηx+η2)ssssss+152c1a1(q2x∂x-1ηy+ηx∂x-1ηy+2qx,yηsssssssssssssssss+2ηyη+η2∂x-1ηy)32]+∂y(152c1a1η2x)=0.It may be noticed that (56) is not a Riccati-type equation. Similar to [27], inserting expansion
(58)η=ε+∑n=1∞‍In(q,qx,qy,…)ε-ninto (56) would lead to
(59)∑n=1∞In,2xε-n+3(ε+∑n=1∞Inε-n)(q2x+∑n=1∞In,xε-n)+3ε2∑n=1∞Inε-n+3ε(∑n=1∞Inε-n)2+(∑n=1∞Inε-n)3+c1∑n=1∞∂x-1In,yε-n=0;collecting the coefficients for the power ofε, we explicity obtain the recursion relations for the conserved densities In′s:
(60)I1=-q2x,I2=q3x,I3=-13(2q4x-c1qx,y),I4=13(q5x-2c1q2x,y),⋮,In+1=-13(∑i+j+k=n-1‍In-1,2x+3In,x+3q2xIn-1+3∑k=1n-2‍IkIn-1-k,x+3∑k=1n-1‍IkIn-k+∑i+j+k=n-1IiIjIk+c1∂x-1In-1,y‍),(n≥4).Applying (58) to divergence-type equation (57) and comparing the power of ε provide us with an infinite sequence of conservation laws:
(61)In,t+Fn,x+Gn,y=0,(n=1,2,…),where the first fluxesFn′s are given explicitly by
(62)F1=-q6xa1+52c1a1q3x,y-15a1q2x3-15c1a1q2xqx,y+5c12a1q2y-15a1q2xq4x,⋮,Fn=-32a1[In,4x+5q4xIn+5∑k=1n-1‍Ik,3xIn-kssssssssss+5In+1,3x+10q2xIn,2xssssssssss+10∑k=1n-1‍Ik,xIn-k,2x+10In+2,2xssssssssss+20∑k=1n‍IkIn+1-k,2x+10∑i+j+k=n‍IiIjIk,2xssssssssss+15q2x2In+30q2x(∑k=1n-1‍Ik,xIn-k+In+1,x)ssssssssss+15∑i+j+k=n‍Ii,xIj,xIk+15∑k=1nIk,xIn+1-k,xssssssssss+10q2x(∑i+j+k=n‍IiIjIk+3∑k=1n‍IkIn+1-k+3In+2)ssssssssss+10∑i+j+k+l=n‍Ii,xIjIkIl+30∑i+j+k=n+1‍Ii,xIjIkssssssssss+30∑k=1n+1‍Ik,xIn+2-k+10In+3,xssssssssss+∑i+j+k+l+m=n‍IiIjIkIlIm+5∑i+j+k+l=n+1‍IiIjIkIlssssssssss+10∑i+j+k=n+2‍IiIjIk+10∑k=1n+2‍IkIn+3-k+5In+4]-152a1(In+3,x+∑k=1n+2‍IkIn+3-k+2In+4)+152c1a1(q2x∂x-1In,y+∑k=1n-1‍∂x-1Ik,yIn-k,xssssssssssssss+2qx,yIn+2In+1,y+2∑k=1n-1‍In-k,yIkssssssssssssss+∑i+j+k=n‍IiIj∂x-1Ik,yssssssssssssss+2∑k=1n‍∂x-1Ik,yIn+1-k+∂x-1In+2,y),and the second fluesGn′s are
(63)G1=-152c1a1q4x,⋮,Gn=152c1a1In,2x,n=2,3,….With the recursion formulae (60), (62), and (63) presented above, the infinite conservation laws for (2) can be constructed. In particular, the first conservation law is
(64)q2x,t+a1q7x+15a1q3xq4x+15a1q2xq5x+45a1q2x2q3x-5c12a1qx,2y+15c1a1q3xqx,y+15c1a1q2xq2xq2x,y=0,or equivalently(65)ut+a1u5x+15a1c0e∫‍a9dtuxu2x+15a1c0e∫‍a9dtuu3x+45a1c02e2∫‍a9dtu2ux+5c1a1u2x,y-5c12a1∂x-1u2y+15c1a1c0e∫‍a9dtux∂x-1uy+15c1a1c0e∫‍a9dtuuy+a9u=0,which is exactly (2) under the constraint conditions (29).


## 6. Conclusion

In this paper, a (2 + 1)-dimensional variable-coefficient CDGKS equation has been investigated by the Bell polynomials approach. For case 1, the CDGKS equation is completely integrable in the sense that it admits bilinear BT, Lax pair, and infinite conservation laws which are derived in a direct and systematic way. By means of the bilinear equation, theN-soliton solutions for the variable-coefficient CDGKS equation are presented. Different parameters and functions are selected to obtain some soliton solutions and also analyze their graphics in Figures 1–3. However, for case 2, the variable-coefficient CDGKS equation under the constraint conditions (37) is not integrable since its multisoliton solutions cannot be obtained. In addition, the integrable constraint conditions on variable coefficients of the equation can be naturally found in the procedure of applying the Bell polynomials approach.



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*Source: 523136-2014-10-14.xml*