Research article

Economic policy uncertainty and stock returns—evidence from the Japanese market

  • Received: 07 April 2020 Accepted: 15 June 2020 Published: 18 June 2020
  • JEL Codes: G11, G12, G15

  • This study examines the impact of changes in economic policy uncertainty (?EPU) on the Japanese (excess) stock return. Evidence of a negative?EPU coefficient implies that heightened economic policy uncertainty (EPU) will cause a decline in stock returns; however, a positive effect in the lagged coefficient of EPU suggests an increase in stock returns. This phenomenon also displays with a rise in uncertainties for fiscal policy, monetary policy, trade policy, global EPU or total uncertainty in Japanese market. Testing of asymmetrical impacts for an upward or downward shift in uncertainty indicates the presence of inverse relations between uncertainty changes and stock returns. Yet, the degree of asymmetry of uncertainty changes on stock returns is more significant from the Japanese own market as compared with U.S. influence.

    Citation: Thomas C. Chiang. Economic policy uncertainty and stock returns—evidence from the Japanese market[J]. Quantitative Finance and Economics, 2020, 4(3): 430-458. doi: 10.3934/QFE.2020020

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  • This study examines the impact of changes in economic policy uncertainty (?EPU) on the Japanese (excess) stock return. Evidence of a negative?EPU coefficient implies that heightened economic policy uncertainty (EPU) will cause a decline in stock returns; however, a positive effect in the lagged coefficient of EPU suggests an increase in stock returns. This phenomenon also displays with a rise in uncertainties for fiscal policy, monetary policy, trade policy, global EPU or total uncertainty in Japanese market. Testing of asymmetrical impacts for an upward or downward shift in uncertainty indicates the presence of inverse relations between uncertainty changes and stock returns. Yet, the degree of asymmetry of uncertainty changes on stock returns is more significant from the Japanese own market as compared with U.S. influence.


    Studying of exact solutions plays a vital role in revealing various mathematical and physical features of associated nonlinear evolution equations (NLEEs). There are diverse types of physically important exact solutions, such as soliton solutions, rational solutions, positons and complexiton solutions. Soliton solutions are a type of analytic solutions exponentially localized[1,2]. Positon solutions contain only one class of transcendental functions-trigonometric functions, while complexiton solutions contain two classes of transcendental functions-exponential functions and trigonometric functions [3,4,5]. Such exact solutions have been explored owing to various specific mathematical techniques, including the Hirota bilinear approach [6,7,8], the extended transformed rational function technique [9], the symbolic computation method [10] and the Wronskian technique [11,12,13,14]. Among the existing methods, the Wronskian technique is widely used to construct exact solutions of bilinear differential equations, particularly rational solutions and complexiton solutions [3,4,5].

    The standard Korteweg-de Vries (KdV) equation and the nonlinear Schrödinger (NLS) equation are two of the most famous integrable models in (1+1)-dimensions which possess very wide applications in a number of fields of nonlinear science. It is known that the KdV equation is applied to describing one-dimensional water waves of long wavelength and small amplitude on shallow-water waves with weakly non-linear restoring forces [15]. The NLS equation is also an interesting mathematical model that describes the motion of pulses in nonlinear optical fibers and of surface gravity waves in fluid dynamics. To explore abundant complex nonlinear phenomena in the real world, various (1+1)-dimensional extensions associated with the KdV and the NLS equations were constructed [16,17,18,19,20,21], including the time-fractional coupled Schrödinger-KdV equation [17] and the coupled nonlinear Schrödinger-KdV equation [19].

    Just recently a novel integrable (2+1)-dimensional KdV equation

    ut=a(6uux+uxxx3wy)+b(2wuxzy+uxxy+4uuy), uy=wx, uyy=zxx, (1.1)

    has been systematically proposed as a two-dimensional extension of the standard KdV equation by Lou [22]. The Lax pair and dual Lax pair presented directly guarantee the integrability of Eq (1.1) [22]. More significantly, the missing D'Alembert type solutions and the soliton molecules have been obtained explicitly through the velocity resonant mechanism and the arbitrary traveling wave solutions, respectively.

    The above-mentioned research inspires us to consider a new generalization of Eq (1.1), written as

    a(6χuux+uxxx+3δvxy)+b(uxxy+2χuxvx+4χuuy+δvyy)+cut+dux+huy=0, vxx=uy, (1.2)

    where the constants a,b,c,χ and δ satisfy χδc(a2+b2)0, but the constants d and h are arbitrary. Equation (1.2) can provide us with some integrable equations in (2+1)-dimensions to model the motion of two-dimensional nonlinear solitary waves in various science fields, such as plasma physics, fluid dynamics and nonlinear optics. Special physically important cases of Eq (1.2) have been investigated as follows:

    If we take χ=1,δ=c=1,d=h=0 and vx=w, Eq (1.2) reduces to the integrable (2+1)-dimensional KdV Eq (1.1). Equation (1.1) may be found potential applications in nonlinear science due to the existence of diverse solution structures [22].

    If we set χ=b=1,δ=1,a=d=h=0,c=2 and make use of the potential u=Ψx, Eq (1.2) is expressed as

    Ψxxxxy+4ΨxxyΨx+2ΨxxxΨy+6ΨxyΨxxΨyyy2Ψxxt=0, (1.3)

    which is the Date-Jimbo-Kashiwara-Miwa (DJKM) equation in (2+1)-dimensions [23,24]. The (2+1)-dimensional DJKM equation is one of the significant integrable models which possesses interesting properties, such as the bilinear Bäcklund transformation, Lax pairs and infinitely many conservation laws [23,24,25].

    Setting χ=1,δ=α2,a=h=0,b=c=1,d=β2 and using the potential u=Φx in Eq (1.2) yield the following extended Bogoyavlenskii's generalized breaking soliton equation introduced by Wazwaz [26]:

    (Φxt4ΦxΦxy2ΦyΦxx+Φxxxy)x=α2Φyyyβ2Φxxx, (1.4)

    where the parameters α2 and β2 are real. Multiple soliton solutions have been derived for Eq (1.4) by applying the simplified Hereman's method.

    We take

    b=h=0, a=s3, c=s1, d=α1, δ=s43s3, χ=s23s3,

    then Eq (1.2) becomes the extended Kadomtsev-Petviashvili (KP) equation discussed by Akinyemi [27] as follows:

    s1utx+α1uxx+s2(u2)xx+s3uxxxx+s4uyy=0, (1.5)

    where the constants s1s4 and α1 satisfy s1s2s3s4α10. Abundant exact solutions including the shallow ocean wave solitons, Peregrine solitons, lumps and breathers solutions have been obtained in [27], which implicates Eq (1.5) might well be applied to explaining a variety of complex behaviors in ocean dynamics.

    The main purpose of this paper is to construct abundant exact solutions including linear superposition solutions, soliton solutions and more importantly their interaction solutions for Eq (1.2). Note that Eq (1.2) has a trilinear form rather than the usual bilinear form [6]. Our work will provide a comprehensive way for building linear superposition solutions and Wronskian interaction solutions.

    The following is the structure of the paper. In Section 2, on the basis of the bilinear Bäcklund transformation, we would like to derive a Lax pair and linear superposition solutions, which can contain some special linear superposition solutions. In Section 3, we will present a set of sufficient conditions which guarantees the Wronskian determinant is a solution of the trilinear form associated with Eq (1.2). And then we will construct a few special but meaningful Wronskian solutions, including N-soliton solutions and novel interaction solutions among different types Wronskian solutions. Our concluding remarks will be drawn in the last section.

    Under the logarithmic derivative transformation

    u=2χ(lnf)xx, v=2χ(lnf)y, (2.1)

    we transformed the extended Eq (1.2) into a trilinear form

    a(f2fxxxxx+2ffxxfxxx5ffxfxxxx6f2xxfx+8fxxxf2x+3δf2fxyy3δffxfyy 
    6δffyfxy+6δfxf2y)+b(f2fxxxxyffxxxxfy+2ffxxfxxy4ffxfxxxy
    +4fxfxxxfy2f2xxfy4fxxfxfxy+4f2xfxxy+δf2fyyy+2δf3y3δffyfyy)
    +c(f2fxxtffxxft2ffxfxt+2f2xft)+d(f2fxxx3ffxfxx+2f3x)
    +h(f2fxxyffxxfy2ffxfxy+2f2xfy)=0.    (2.2)

    It is known that Hirota bilinear derivatives with multiple variables read:

    Dn1xDn2tfg=(xx)n1(tt)n2f(x,t)g(x,t)|x=x,t=t, (2.3)

    with n1 and n2 being arbitrary nonnegative integers [6]. By utilizing Hirota bilinear expressions, we can rewrite the trilinear form (2.2) as

    Dx[(3aD4x+9aδD2y+2bD3xDy+3cDxDt+3dD2x+3hDxDy)ff]f2
    +Dy[(bD4x+3bδD2y)ff]f2=0.  (2.4)

    Theorem 2.1. Assume that f and f are two different solutions of Eq (2.2). Then we can give the following bilinear Bäcklund transformation of (2.2):

    (˜δDy+D2x)ff=0, (2.5a)
    [aD3x+bD2xDy3a˜δDxDyb˜δD2y+cDt+dDx+hDy]ff=0, (2.5b)

    where ˜δ2=δ.

    By the same calculation introduced in [23,24,28], we would like to present a simple proof of Theorem 2.1 in Appendix A.

    Setting

    ψ=ff,u=2χ(lnf)xx, (2.6)

    and using the identities of double logarithmic transformations [6]

    {(Dxff)/f2=ψx,(D2xff)/f2=ψxx+χuψ,(D3xff)/f2=ψxxx+3χuψx,(DxDyff)/f2=ψxy+χ1xuyψ,(D2xDyff)/f2=ψxxy+2χ1xuyψx+χuψy,,

    we can transform the bilinear Bäcklund transformation (2.5) into a Lax system of Eq (1.2) as follows:

    L1ψ=˜δψy+ψxx+χuψ=0, (2.7a)
    L2ψ=cψt2b˜δψxxxx+4aψxxx(4bχ˜δu+h˜δ)ψxx+2(3aχu2bχ˜δux+bχ1xuy+d2)ψx
         (3aχ˜δ1xuy+bχ˜δ2xu2y+2bχ2˜δu23aχux+2bχ˜δuxxbχuy+h˜δχu)ψ=0, (2.7b)

    where

    L1=˜δy+2x+χu,  (2.8a)
    L2=ct2b˜δ4x+4a3x(4bχ˜δu+h˜δ)2x+2(3aχu2bχ˜δux+bχ1xuy+d2)x
    (3aχ˜δ1xuy+bχ˜δ2xu2y+2bχ2˜δu23aχux+2bχ˜δuxxbχuy+h˜δχu). (2.8b)

    Note that Eq (1.2) can be generated from the compatibility condition [L1,L2]=0 of the system (2.7), which represents the integrability of Eq (1.2).

    In addition, taking f=1 as the seed solution in the system (2.5), we further obtain the following linear partial differential equations:

    ˜δfy+fxx=0, (2.9a)
    afxxx+bfxxy3a˜δfxyb˜δfyy+cft+dfx+hfy=0, (2.9b)

    which is rewritten as

    ˜δfy+fxx=0, (2.10a)
    4afxxx2b˜δfxxxx+cft+dfxh˜δfxx=0. (2.10b)

    It is easy to see that the system (2.7) with the choice u=0 is equivalent to the the pair of Eq (2.10). Generally, the linear superposition principle can not be directly applied to solutions of NLEEs. However, it is widely known that the linear superposition principle of solutions [29,30,31,32] can be applied to homogeneous linear differential equations. Therefore, solving the system (2.10) above, we can built a linear superposition solution formed by linear combinations of exponential functions as follows:

    f=Ni=1εieθi+θ0i,θi=kix1˜δk2iy+(2b˜δck4i4ack3i+h˜δck2idcki)t, (2.11)

    where the ki,s are arbitrary non-zero constants, the ε,is, θ0i,s are arbitrary constants and ˜δ satisfies ˜δ2=δ. The following are two cases which are composed of the product of two special functions for the trilinear form (2.2).

    (a) The case of δ>0:

    If we choose

    ki=ri+li, θ0i=θ0i1+θ0i2

    and

    ki=rili, θ0i=θ0i1θ0i2, ri,li,θ0i1,θ0i2R, 1iN,

    then the linear superposition solution (2.11) becomes

    f=Ni=1εieθi1eθi2andf=Ni=1εieθi1eθi2,

    with N-wave variables

    θi1=rix1˜δ(r2i+l2i)y+[2b˜δc(r4i+6r2il2i+l4i)4ac(r3i+3ril2i)+h˜δc(r2i+l2i)dcri]t+θ0i1,
    θi2=lix2˜δriliy+[8b˜δc(r3ili+ril3i)4ac(3r2ili+l3i)+2h˜δcrilidcli]t+θ0i2, (2.12)

    respectively. Therefore, two kinds of linear superposition formulas of Eq (2.2) composed of the product of exponential functions and hyperbolic functions can be expressed as

    f=Ni=1εieθi1cosh(θi2),f=Ni=1εieθi1sinh(θi2), (2.13)

    where θi1 and θi2 are defined by (2.12).

    By setting

    ki=ri+Ili, θ0i=θ0i1+Iθ0i2

    and

    ki=riIli, θ0i=θ0i1Iθ0i2, ri,li,θ0i1,θ0i2R, I=1, li0, 1iN,

    respectively, we have

    f=Ni=1εieRe(θi)eI×Im(θi)andf=Ni=1εieRe(θi)eI×Im(θi),

    where

    Re(θi)=rix1˜δ(r2il2i)y+[2b˜δc(r4i6r2il2i+l4i)4ac(r3i3ril2i)+h˜δc(r2il2i)dcri]t+θ0i1,
    Im(θi)=lix2˜δriliy+[8b˜δc(r3iliril3i)4ac(3r2ilil3i)+2h˜δcrilidcli]t+θ0i2. (2.14)

    Thus two classes of solutions formed by the product of exponential functions and trigonometric functions appear as:

    f=Ni=1εieRe(θi)cos(Im(θi)), f=Ni=1εieRe(θi)sin(Im(θi)), (2.15)

    with Re(θi) and Im(θi) being given by (2.14). Besides, applying the linear superposition principle, we may get the following mixed-type function solutions such as complexiton solutions:

    f=Ni=1[εieθi+ϱieRe(θi)sin(Im(θi))],f=Ni=1[εieθi+ϱieRe(θi)cos(Im(θi))], (2.16)

    where the ε,is, ϱ,is are arbitrary constants, θi and Re(θi), Im(θi) are defined by (2.11) and (2.14), respectively.

    (b) The case of δ<0:

    Generally, the above solution (2.11) leads to complex-valued linear combinations if δ<0. However, we are more interested in real solutions. To this end, taking

    ki=Iri+li, θ0i=Iθ0i1+θ0i2

    and

    ki=Irili, θ0i=Iθ0i1θ0i2, ri,li,θ0i1,θ0i2R, I=1, li0, 1iN,

    in (2.11), respectively, we get the following two types of solutions of Eq (2.2):

    f=Ni=1εieIκieςiandf=Ni=1εieIκieςi,

    with N-wave variables

    κi=rix1δ(r2il2i)y+[2bδc(6r2il2ir4il4i)+4ac(r3i3ril2i)+hδc(r2il2i)dcri]t+θ0i1,
    ςi=lix2δriliy+[8bδc(ril3ir3ili)+4ac(3r2ilil3i)+2hδcrilidcli]t+θ0i2. (2.17)

    Similarly, the following linear superposition formulas:

    f=Ni=1εieIκicosh(ςi), f=Ni=1εieIκisinh(ςi), (2.18)

    with κi and ςi being defined by (2.17), solve the linear partial differential system (2.10). Let N=1 in the solution (2.18). Through the transformation (2.1), a real solution of Eq (1.2) reads as

    u=8l21e2ς1χ(1+e2ς1)2, vx=16l21r1e2ς1χδ(1+e2ς1)2, (2.19)

    with ς1 being defined by (2.17), which is nothing but the one-soliton solution of Eq (1.2).

    Let us take the extended Bogoyavlenskii's generalized breaking soliton Eq (1.4) with α2>0 as an illustrative example to describe the propagations of linear superposition solutions. By the transformation (2.1), we have the following special N-order linear superposition solutions for Eq (1.4) with α2>0:

    Φ=2(lnf)x, f=Ni=1εiekix1αk2iy+(2αk4iβ2ki)t, (2.20)
    Φ=2(lnf)x, 
    f=Ni=1εierix1α(r2i+l2i)y+[2α(r4i+6r2il2i+l4i)β2ri]t×cosh(lix2αriliy+[8α(r3ili+ril3i)β2li]t), (2.21)

    and

    Φ=2(lnf)x,
      f=Ni=1[εiekix1αk2iy+(2αk4iβ2ki)t+ϱierix1α(r2il2i)y+[2α(r4i6r2il2i+l4i)β2ri]t
    ×cos(lix2αriliy+[8α(r3iliril3i)β2li]t)], (2.22)

    where the ε,is, ϱ,is, k,is r,is and l,is are arbitrary real constants.

    Three-dimensional plots of these linear superposition solutions are made with the aid of Maple plot tools, to depict the characteristics of linear superposition solutions. The solution (2.20) is a linear combination of N exponential wave solutions, also known as the N-wave solution [29]. Figure 1(a)(c) displays that the three-dimensional plots of the linear superposition solution (2.20) for N=4,N=5 and N=6 and correspondingly presents three-wave, four-wave and five-wave, respectively.

    Figure 1.  Three-dimensional plots of Φ determined by the linear superposition solution (2.20) with special parameters: (a) N = 4, εi=1,1i4,k1=1.2,k2=0.5,k3=1.8,k4=3,α=1,β=2,t=0; (b) N = 5, εi=1,1i5,k1=1.2,k2=0.5,k3=1.8,k4=3,k5=0.5,α=1,β=2,t=0; (c) N = 6, εi=1,1i6,k1=1.2,k2=0.5,k3=1.8,k4=3,k5=0.5,k6=2,α=1,β=2,t=0.

    Figure 2(a)(c) displays the two-dimensional density plots corresponding to Figure 1(a)(c). We can see from Figures 1 and 2 that the solution (2.20) manifests a kink-shape traveling wave in the (x,y)-plane and the number of stripes increases with the increase of the positive integer N at t=0. In addition, various phenomena of wave fusion or fission may occur when the traveling multi-kink waves propagate along different or same directions. If the coefficients ε,is are all positive real constants, then the f in the solutions (2.20) and (2.21) is a positive function. But the coefficients ε,is and ϱ,is are all positive real constants can not guarantee that the function f is always positive in the complexiton solution (2.22).

    Figure 2.  Two-dimensional density plots of Φ determined by the linear superposition solution (2.20). The related parameters are the same as in Figure 1.

    Figure 3 shows three-dimensional graphics of the complexiton solutions, which possessing some singularities. It is obvious that the evolution of linear superposition solutions inclines to be more complicated with the increase of the positive integer N.

    Figure 3.  Three-dimensional plots of Φ determined by the linear superposition solution (2.22) with special parameters: (a) N = 2, ε1=ε2=1,ϱ1=ϱ2=1,k1=1,k2=2,r1=1,l1=2,r2=3,l2=1,α=1,β=2,t=0; (b) N = 3, εi=1,1i3,ϱ1=1,ϱ2=ϱ3=0,k1=1,k2=1.5,k3=2.5,r1=1,l1=2,α=1,β=2,t=0; (c) N = 3, εi=1,ϱi=1,1i3,k1=1,k2=3,k3=0.5,r1=1,l1=2,r2=3,l2=1,r3=1,l3=1.5,α=1,β=2,t=0.

    Based on the pair of Eq (2.10), we now construct a set of sufficient conditions on Wronskian solutions for the extended (2+1)-dimensional KdV Eq (1.2). We first introduce the compact Freeman and Nimmo's notation [12,13]:

    W=W(ϕ1,ϕ2,,ϕN)=|ϕ1ϕ(1)1ϕ(N1)1ϕ2ϕ(1)2ϕ(N1)2ϕNϕ(1)Nϕ(N1)N|=|0,1,,N1|=|^N1|, (3.1)

    where ϕ(j)i=jϕixj,i,j1. Then we present a set of sufficient conditions, which guarantees that the Wronskian determinant is a solution of the trilinear Eq (2.2).

    Theorem 3.1. Suppose that a set of functions ϕi=ϕi(x,y,t),1iN, meets the combined linear conditions as follows:

    ϕi,y=1˜δϕi,xx, (3.2a)
    ϕi,t=2b˜δcϕi,xxxx4acϕi,xxx+h˜δcϕi,xxdcϕi,x, (3.2b)

    where ˜δ2=δ. Then the Wronskian determinant f=fN=|^N1| defined by (3.1) solves the trilinear Eq (2.2).

    The proof of Theorem 3.1 will be presented by using Wronskian identities of the bilinear KP hierarchy in Appendix B. We can check that the above sufficient conditions reduce to the ones introduced earlier studies for the (2+1)-dimensional DJKM Eq (1.3) [33,34].

    It is known that Wronskian formulations provide us with a powerful technique to establish exact solutions including soliton solutions, rational solutions, positons, complexitons and their interaction solutions for NLEEs [3,4,5]. The interactions of mixed solutions for higher-dimensional NLEEs have become a more and more popular research topic recently [35,36,37,38,39,40,41]. The determination of mixed solutions is extremely useful to reveal specific physical characteristics modeled by these higher-dimensional equations. With the help of the homoclinic test method and the Hirota bilinear approach, different types of hybrid-type solutions were displayed, such as the breather-kink wave solutions [36], the mixed lump-kink solutions [37] and the periodic-kink wave solutions [38]. In this section, the major concern is to construct Wronskian interaction solutions among different types of Wronskian solutions determined by the set of Wronskian sufficient condition (3.2) to the trilinear Eq (2.2).

    Let us consider the Wronskian sufficient condition (3.2). An N-soliton solution of Eq (2.2) associated with the Wronskian determinant can be expressed as

    f=fN=W(ϕ1,ϕ2,,ϕN), (3.3)

    where

    ϕi=eξi+e^ξi,ξi=pix1˜δp2iy+(2b˜δcp4i4acp3i+h˜δcp2idcpi)t+constant,
    ^ξi=qix1˜δq2iy+(2b˜δcq4i4acq3i+h˜δcq2idcqi)t+constant, (3.4)

    in which p,is and q,is are free parameters. Taking the variables transformations presented in [6] and introducing the following new parameters:

    Ki=piqi,Li=1˜δ(p2iq2i),Wi=2b~δc(p4iq4i)4ac(p3iq3i)+h˜δc(p2iq2i)dc(piqi), (3.5)

    the dispersion relation of Eq (2.2) can be written as

    Wi=acKi(3δL2i+K4i)bcK2i(δL3i+K4iLi)dKichLic. (3.6)

    Moreover, through the same calculation and variables transformations presented in [34], we obtain an equivalent representation of the N-soliton solution (3.3) as follows:

    f=fN=μ=0,1eN1i<jμiμjlnAij+Ni=1μiηi, (3.7)

    where

    ηi=Kix+Liy+Wit+η0i, Aij=K2iK2j(KiKj)2+δ(KiLjKjLi)2K2iK2j(Ki+Kj)2+δ(KiLjKjLi)2,1i<jN, (3.8)

    with Wi being defined by (3.6) and η0i's being arbitrary constants. Here μ=(μ1,μ2,,μN), μ=0,1 indicates that each μi takes 0 or 1. Also worth noting is that if we choose all the Aij=0, the N-soliton solution (3.7) can be reduced to the linear superposition solution (2.11).

    Next we will show different types of Wronskian interaction solutions to Eq (1.2). In general, it will lead to complex-valued Wronskian interaction solutions when δ<0. For the convenience of the following discussion, we will only focus on the case of δ>0 in Eq (1.2).

    Solving the following representative system

    ϕy=1˜δϕxx, (3.9a)
    ϕt=2b˜δcϕxxxx4acϕxxx+h˜δcϕxxdcϕx, (3.9b)

    with ˜δ2=δ>0, we get several special solutions for ϕ :

    ϕrational,1=α1xdα1ct+α2,α1,α2=constants, (3.10a)
    ϕrational,2=β1x2+β2x2β1˜δy+2β1hc˜δt+β3,d=0,β1,β1,β3=constants, (3.10b)
    ϕsoliton=eξ+eˆξ,ξ=px1˜δp2y+(2b˜δcp44acp3+h˜δcp2dcp)t,  
    ˆξ=qx1˜δq2y+(2b˜δcq44acq3+h˜δcq2dcq)t,p,q=constants, (3.10c)
    ϕpositon,1=eˆφcosφ, ϕpositon,2=eˆφsinφ, ϕcomplexiton=eξ+eˆφcosφ,  
    ξ=px1˜δp2y+(2b˜δcp44acp3+h˜δcp2dcp)t,     
        ˆφ=rx1˜δ(r2l2)y+[2b˜δc(r46r2l2+l4)4ac(r33rl2)+h˜δc(r2l2)dcr]t,
      φ=lx2˜δrly+[8b˜δc(r3lrl3)4ac(3r2ll3)+2h˜δcrldcl]t,p,r,l=constants. (3.10d)

    A few Wronskian interaction determinants between any two of a single soliton, a rational, a positon and a complexiton read as

    f=W(ϕrational,1,ϕsoliton)=eˆξ[α1q(α1xdα1ct+α2)+(α1p(α1xdα1ct+α2))eξˆξ],
    f=W(ϕrational,2,ϕsoliton)=eˆξ[2β1x+β2q(β1x2+β2x2β1˜δy+2β1hc˜δt+β3)
    +(2β1x+β2p(β1x2+β2x2β1˜δy+2β1hc˜δt+β3))eξˆξ], d=0,
    f=W(ϕrational,1,ϕpositon,1)=eˆφ[(α1xdα1ct+α2)(rcosφlsinφ)α1cosφ],   
    f=W(ϕsoliton,ϕpositon,2)=eˆξ+ˆφ[(1+eξˆξ)(rsinφ+lcosφ)(peξˆξ+q)sinφ],   
    f=W(ϕrational,1,ϕcomplexiton)=(α1xdα1ct+α2)(peξ+reˆφcosφleˆφsinφ)α1(eξ+eˆφcosφ),

    where ξ,ˆξ and φ,ˆφ are defined by (3.10c) and (3.10d), respectively. Moreover, by the transformation (2.1), the corresponding Wronskian interaction solutions of Eq (1.2) appear as

    u=2(ffxxf2x)χf2, vx=2(ffxyfxfy)χf2. (3.11)

    For Eq (1.4) with α2>0, associated with (3.11), three special Wronskian interaction solutions are

    Φrs=2xlnW(ϕrational,1,ϕsoliton)=2q2ˉfrs,xˉfrs,   (3.12)
    ˉfrs=α1q(α1xβ2α1t+α2)+[α1p(α1xβ2α1t+α2)]eξˆξ,   
    ˉfrs,x=qα1+[pα1+(α1p(α1xβ2α1t+α2))(pq)]eξˆξ,
    Φrp=2xlnW(ϕrational,1,ϕpositon,1)=2r2ˉfrp,xˉfrp, (3.13)
    ˉfrp=(α1xβ2α1t+α2)(rcosφlsinφ)α1cosφ,  
    ˉfrp,x=α1(rcosφlsinφ)(α1xβ2α1t+α2)(rlsinφ+l2cosφ)+α1lsinφ,
    Φsp=2xlnW(ϕsoliton,ϕpositon,2)=2(q+r)2ˉfsp,xˉfsp,    (3.14)
    ˉfsp=(1+eξˆξ)(rsinφ+lcosφ)(peξˆξ+q)sinφ,
    ˉfsp,x=eξˆξ(pq)(rsinφ+lcosφ)+(1+eξˆξ)(rlcosφl2sinφ)
    eξˆξp(pq)sinφ(peξˆξ+q)lcosφ,

    where

    ξˆξ=(pq)x1α(p2q2)y+2α(p4q4)tβ2(pq)t,
      φ=lx2αrly+8α(r3lrl3)tβ2lt,α1,α2,p,q,r,l=constants.

    Figure 4 shows some singularities of these three Wronskian interaction solutions.

    Figure 4.  (a) The plot of the Wronskian interaction solution (3.12) with parameters: p=1,q=3,α1=2,α2=0,α=1,β=2,t=0; (b) The plot of the Wronskian interaction solution (3.13) with parameters: r=2,l=1,α1=1,α2=2.1,α=1,β=2,t=0; (c) The plot of the Wronskian interaction solution (3.14) with parameters: p=1,q=3,r=1,l=2,α=1,β=2,t=0.

    In a word, on the basis of the bilinear Bäcklund transformation, we established a Lax system and linear superposition solutions composed of exponential functions for the trilinear Eq (2.2). Furthermore, by extending the involved parameters to the complex field, we obtained some special linear superposition solutions, such as the linear superposition formula of the product of exponential functions and trigonometric functions, the linear superposition formula of the product of exponential functions and hyperbolic functions, and the mixed-type function solutions. Finally, a set of sufficient conditions, which guarantees that the Wronskian determinant is a solution of Eq (2.2), was given associated with the bilinear Bäcklund transformation. The resulting Wronskian structure generated the N-soliton solution and a few special Wronskian interaction solutions for Eq (1.2).

    In a sense, the presented results in this paper extend existing studies, because many soliton equations can be used as special cases of Eq (1.2). The bilinear Bäcklund transformation (2.5) and Lax system (2.7) indicate the integrability of Eq (1.2). By employing Wronskian identities of the bilinear KP hierarchy and properties of Hirota operators, we provide a direct and simple verification of the Wronskian determinant solution, which avoids a lengthy and complex proof process. Our studies also demonstrate the diversity and richness of solution structures of the introduced equation.

    We remark that Eq (1.2) possesses a kind of traveling wave solutions in the form:

    u=2χ(lng(τ))xx, v=2χ(lng(τ))y, τ=xaby(2δa3cb2+dcahbc)t+τ0,

    where the coefficients a and b are two nonzero constants, g is an arbitrary function and τ0 is an arbitrary constant.

    Therefore Eq (1.2) has a large number of solution formulas including soliton molecules [22,42]. Furthermore, in our future work, lump solutions [10,34,43,44,45] and nonsingular complexiton solutions [10] are expected to be studied for Eq (1.2) with δ<0. These wonderful solutions will be useful for analyzing nonlinear phenomena in realistic applications.

    The authors express their sincere thanks to the referees and editors for their valuable comments. This work is supported by the National Natural Science Foundation of China (No.12271488) and Jinhua Polytechnic Key Laboratory of Crop Harvesting Equipment Technology of Zhejiang Province.

    The authors declare that they have no known competing financial interest or personal relationships that could have appeared to influence the work reported in this paper.

    We provide a simple proof of Theorem 2.1.

    Proof. Let us start from a key function

    P=f4{Dx[(3aD4x+9aδD2y+2bD3xDy+3cDxDt)ff]f2
    +Dy[(bD4x+3bδD2y)ff]f2}f4{Dx[(3aD4x+9aδD2y   
    +2bD3xDy+3cDxDt)ff]f2+Dy[(bD4x+3bδD2y)ff]f2}.  (A.1)

    By applying (2.5a) and Theorem 2.1 obtained in [28], we have

    P=6Dx{Dx[(aD3x+bD2xDy3a˜δDxDyb˜δD2y+cDt)ff]ff}f2f2. (A.2)

    Let us introduce another key function

    Q=f4{Dx[(3dD2x+3hDxDy)ff]f2}f4{Dx[(3dD2x+3hDxDy)ff]f2}. (A.3)

    By employing the folllowing exchange identities for Hirota's bilinear operators [6]:

    (DxFG)H2G2(DxTH)=Dx(FHGT)GH, (A.4a)
    (DyDxFF)G2F2(DyDxGG)=2Dx(DyFG)FG=2Dy(DxFG)FG, (A.4b)

    a direct computation shows

    Q=Dx{f2(3dD2x+3hDxDy)fff2(3dD2x+3hDxDy)ff}f2f2
    =6Dx{Dx[(dDx+hDy)ff]ff}f2f2. (A.5)

    It further follows that

    P+Q=f4{Dx[(3aD4x+9aδD2y+2bD3xDy+3cDxDt+3dD2x+3hDxDy)ff]f2
    +Dy[(bD4x+3bδD2y)ff]f2}f4{Dx[(3aD4x+9aδD2y+2bD3xDy   
    +3cDxDt+3dD2x+3hDxDy)ff]f2+Dy[(bD4x+3bδD2y)ff]f2}   
            =6Dx{Dx[(aD3x+bD2xDy3a˜δDxDyb˜δD2y+cDt+dDx+hDy)ff]ff}f2f2. (A.6)

    Thus, the system of bilinear Eq (2.5) guarantees P+Q=0, which indicates that the system (2.5) yields a Bäcklund transformation for Eq (2.2).

    It is widely known that the first two equations of the KP hierarchy [46] may be expressed in Hirota bilinear form as

    (D414D1D3+3D22)ff=0, (B.1a)
    [(D31+2D3)D23D1D4]ff=0, (B.1b)

    where f denotes a function related to variables xj, j=1,2,3,, and DjDxj. To prove Theorem 3.1, we first give two helpful lemmas in terms of Hirota differential operators.

    Lemma B.1. Suppose that a group of functions ϕi=ϕi(x1,x2,x3,),(1iN), satisfies that

    xjϕi=jϕixj,j=1,2,3,. (B.2)

    Then the Wronskian determinant f=fN=|^N1| defined by (3.1) solves the bilinear Eqs (B.1a) and (B.1b).

    Lemma B.1 has been proved in [6,47]. This lemma demonstrates that the bilinear forms (B.1a) and (B.1b) become the Plücker relations for determinants if the function f is written as the Wronskian determinant [48]. That is, (B.1a) and (B.1b) can be transformed into the following Wronskian identities:

    (D414D1D3+3D22)|^N1||^N1|=24(|^N1||^N3,N,N+1|
    |^N2,N||^N3,N1,N+1|+|^N2,N+1||^N3,N1,N|)0, (B.3a)

    and

    [(D31+2D3)D23D1D4]|^N1||^N1|=12(|^N1||^N3,N,N+2| 
    |^N2,N||^N3,N1,N+2|+|^N2,N+2||^N3,N1,N|)
    12(|^N1||^N4,N2,N,N+1||^N2,N||^N4,N2,N1,N+1| 
    +|^N2,N+1||^N4,N2,N1,N|)0, (B.3b)

    respectively. The first identity (B.3a) is nothing but a Plücker relation, and the second identity (B.3b) is a combination of two Plücker relations.

    Lemma B.2. Let Wronskian entries ϕi=ϕi(x,y,t), 1iN, in the Wronskian determinant (3.1) satisfy (B.2) and

    yϕi=(a1x+a22x++ammx)ϕi(a1x1+a2x2++amxm)ϕi,  (B.4a)
    tϕi=(b1x+b22x++bnnx)ϕi(b1x1+b2x2++bnxn)ϕi, (B.4b)

    where m,n are nonnegative integers, and a1,a2,,am,b1,b2,,bn are arbitrary constants. Then

    f=fN=|^N1|

    defined by (3.1) yields

    Dn1yDn2tff=(a1D1+a2D2++amDm)n1(b1D1+b2D2++bnDn)n2ff, (B.5)

    with n1,n2 are nonnegative integers and DjDxj. The associated Hirota's bilinear operators Dxj,j=1,2,3,, are defined by the expression (2.3).

    Lemma B.2 has been proved in [49]. Next, we present the proof of Theorem 3.1.

    Proof. Introducing an auxiliary variable z, we may rewrite Eq (2.4) as

    Dx[(3aD4x+9aδD2y+2bD3xDy+3cDxDt+3dD2x+3hDxDyDyDz)ff]f2
    +Dy[(bD4x+3bδD2y+DxDz)ff]f2=0.     (B.6)

    Let the Wronskian entries ϕi, 1iN, meets

    ϕi,z=4bϕi,xxx.

    Applying the conditions (3.2) and Lemma B.2, we have

    D4xff=D41ff,D2yff=1δD22ff,D3xDyff=1˜δD31D2ff,
    DxDtff=D1(2b˜δcD44acD3+h˜δcD2dcD1)ff,
    DyDzff=4b˜δD2D3ff,DxDyff=1˜δD1D2ff, 
    DxDzff=4bD1D3ff,.  

    Substituting the above derivatives into (B.6) and employing Lemma B.2, a direct calculation yields

    (3aD4x+9aδD2y+2bD3xDy+3cDxDt+3dD2x+3hDxDyDyDz)ff
    =(3aD41+9aD222b˜δD31D2+6b˜δD1D412aD1D3+3h˜δD1D23dD21
    +3dD213h˜δD1D24b˜δD2D3)ff
       =3a(D41+3D224D1D3)ff2b˜δ(D31D2+2D2D33D1D4)ff
    =0, (B.7)

    and

    (bD4x+3bδD2y+DxDz)ff=b(D41+3D224D1D3)ff=0, (B.8)

    where the Wronskian identities (B.3a) and (B.3b) have been applied. Furthermore, we have

    Dx[(3aD4x+9aδD2y+2bD3xDy+3cDxDt+3dD2x+3hDxDy)|^N1||^N1|]|^N1|2
      +Dy[(bD4x+3bδD2y)|^N1||^N1|]|^N1|2=0.

    Thus, the Wronskian determinant f=fN=|^N1| solves Eq (2.2).



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