
Most of the offshore projects will be impacted by storm surge, especially in the sea area where typhoons are frequent, and storm surge disasters are inevitable. The establishment of a theoretical distribution model of the number of typhoon occurrences and random waves is of great theoretical and practical significance for the study of the number of storm surge impacts and damage to marine engineering as well as the safety evaluation of offshore engineering. Based on stochastic process theory, this paper discusses the effects of the number of typhoon occurrences and typhoon intensity on wave displacement and water level by constructing a compound Poisson process model of typhoon frequency and typhoon intensity. The limitations of using typhoon intensity and wave height as random variables in the marine environment are improved. The average cumulative damage, reliability, and average service life of marine works were analyzed by marine works reliability analysis and a compound Poisson process of the number of storm surge impacts on marine works and the damage caused to marine works by each impact. The results show that the statistical theoretical model and reliability analysis of the storm surge hazard factors based on the stochastic process covers the original extreme value statistical distribution model, and can determine the parameters in the model according to different thresholds in line with the objective facts, and then deduce the design return level, while the deduced return level still has a certain degree of reliability in the case of short or missing data. Therefore, the stochastic process-based model of the imputed level of design parameters for the marine environment provides a new option for marine engineering design and risk management.
Citation: Baiyu Chen, Yi Kou, Yufeng Wang, Daniel Zhao, Shaoxun Liu, Guilin Liu, Liping Wang, Xuefeng Han. Analysis of storm surge characteristics based on stochastic process[J]. AIMS Mathematics, 2021, 6(2): 1177-1190. doi: 10.3934/math.2021072
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Most of the offshore projects will be impacted by storm surge, especially in the sea area where typhoons are frequent, and storm surge disasters are inevitable. The establishment of a theoretical distribution model of the number of typhoon occurrences and random waves is of great theoretical and practical significance for the study of the number of storm surge impacts and damage to marine engineering as well as the safety evaluation of offshore engineering. Based on stochastic process theory, this paper discusses the effects of the number of typhoon occurrences and typhoon intensity on wave displacement and water level by constructing a compound Poisson process model of typhoon frequency and typhoon intensity. The limitations of using typhoon intensity and wave height as random variables in the marine environment are improved. The average cumulative damage, reliability, and average service life of marine works were analyzed by marine works reliability analysis and a compound Poisson process of the number of storm surge impacts on marine works and the damage caused to marine works by each impact. The results show that the statistical theoretical model and reliability analysis of the storm surge hazard factors based on the stochastic process covers the original extreme value statistical distribution model, and can determine the parameters in the model according to different thresholds in line with the objective facts, and then deduce the design return level, while the deduced return level still has a certain degree of reliability in the case of short or missing data. Therefore, the stochastic process-based model of the imputed level of design parameters for the marine environment provides a new option for marine engineering design and risk management.
The Hunter-Saxton (HS) equation reads
uxxt+uuxxx+2uxuxx−2κux=0, | (1.1) |
where u(x,t) depends on a time variable t and a space variable x, κ is a positive constant. This equation was derived as a model for propagation of orientation waves in a massive nematic liquid crystal director field [1]. In fact, it can be regarded as a short wave limit of the well known Camassa-Holm equation [2,3].
The two-component Hunter-Saxton (2-HS) equation [1] is
{uxxt+uuxxx+2uxuxx−2κux=σρρx,ρt+(ρu)x=0, | (1.2) |
where u(x,t) and ρ(x,t) depend on variables t and x, σ,κ are positive constants. The 2-HS equation has attracted much attention and it has been studied extensively and some results were obtained, we can see [4,5].
Meanwhile, there is a generalized 2-HS system [6] as follow:
{uxxt+uuxxx+(1−α)uxuxx−κρρx=0,ρt+uρx=αuxρ, | (1.3) |
where α(α≠1),κ are constants. The model with (α,κ)=(−1,−1) in system (1.3) appeared initially in the work of Lenells [7]. The author showed that system (1.3) is the geodesic equation on a manifold K which admits a K¨ahler structure. The blow-up phenomena of system (1.3) was investigated in [4,8].
Our goal is to study exact solutions of system (1.3) by applying classical Lie group method [9,10,11,12,13,14]. Firstly, the vector field for the system (1.3) will be given by Lie symmetry analysis. Secondly, similarity variables and its symmetry reductions equations are obtained. Thirdly, by solving the reduced equations, some exact solutions of the system (1.3) will be presented. Finally, we give a conservation law of system (1.3).
First of all, let us consider a one-parameter Lie group of infinitesimal transformation:
x→x+ϵξ(x,t,u,ρ), |
t→t+ϵτ(x,t,u,ρ), |
u→u+ϵϕ(x,t,u,ρ), |
ρ→ρ+ϵψ(x,t,u,ρ), |
with a small parameter ϵ≪1. The vector field associated with the above group of transformations can be written as
V=ξ(x,t,u,ρ)∂∂x+τ(x,t,u,ρ)∂∂t+ϕ(x,t,u,ρ)∂∂u+ψ(x,t,u,ρ)∂∂ρ, | (2.1) |
where the coefficient functions ξ(x,t,u,ρ),τ(x,t,u,ρ),ϕ(x,t,u,ρ) and ψ(x,t,u,ρ) of the vector field are to be determined later.
If the vector field (2.1) generates a symmetry of the system (1.3), then V must satisfy the Lie symmetry condition
{pr(3)V(Δ1)|Δ1=0=0,pr(1)V(Δ2)|Δ2=0=0, | (2.2) |
where pr(3)V,pr(1)V denote the third and the first prolongation of V respectively, and Δ1=uxxt+uuxxx+(1−α)uxuxx−κρρx, Δ2=ρt+uρx−αuxρ for system (1.3). Expanding (2.2), we find that the coefficient functions ξ,τ,ϕ and ψ must satisfy the symmetry condition
{ϕxxt+ϕuxxx+uϕxxx+(1−α)ϕxuxx+(1−α)uxϕxx−κψρx−κρψx=0,ψt+ϕρx+uψx−αϕxρ−αuxψ=0, | (2.3) |
where ϕ,ψ,ϕx,ψx,ψt,ϕxx,ϕxxx,ϕxxt are the coefficient functions given by
ϕt=Dtϕ−uxDtξ−utDtτ, ψt=Dtψ−ρxDtξ−ρtDtτ,ϕx=Dxϕ−uxDxξ−utDxτ, ψx=Dxψ−ρxDxξ−ρtDxτ,ϕxx=D2xϕ−uxD2xξ−utD2xτ−2uxxDxξ−2uxtDxτ,ϕxxx=D3xϕ−uxD3xξ−utD3xτ−3uxxD2xξ−3uxtD2xτ−3uxxxDxξ−3uxxtDxτ,ϕxxt=DtD2xϕ−uxDtD2xξ−uxtD2xξ−2uxxDtDxξ−2uxxtDxξ−utDtD2xτ−uttD2xτ−2uxtDtDxτ−2uxttDxτ−uxxxDtξ−uxxtDtτ, | (2.4) |
where Dx,Dt are the total derivatives with respect to x and t respectively.
Substituting (2.4) into (2.3), combined with system (1.3) and setting the coefficients of the various monomials in u and v and their partial derivatives equal to zero one obtains the determining equations for the symmetry group of (1.3) as follows
ξu=0, ξρ=0, τx=0, τu=0, τρ=0, ϕρ=0, ϕuu=0, ϕxxu=0, ψu=0,ρτt+ψ=0, ϕu−ξx−ψρ=0, (1−α)(ϕu−ξx+τt)=0, ξxx−2ϕxu=0,uϕxxx+ϕtxx−κρψx=0, −αρϕx+uψx+ψt=0, −u(ξx−τt)−ξt+ϕ=0,uξxxx−(1−α)ϕxx=0, −2ξtx+(1−α)ϕx+3u(ϕxu−ξxx)+ϕtu=0. | (2.5) |
Solving these determining equations yields
{ξ=(F′1(t)+C1+C2)x+F2(t)+C3,τ=−F1(t)α+C2t+C4,ϕ=F″1(t)x+((1+α)F′1(t)+C1)u+F′2(t),ψ=(αF′1(t)−C2)ρ, | (2.6) |
where F1(t),F2(t) are arbitrary functions of t, C1,C2,C3 and C4 are arbitrary constants.
Thus, the Lie algebra of infinitesimal symmetries of system (1.3) is spanned by the following vector fields
V1=F′1(t)x∂∂x−αF1(t)∂∂t+[F″1(t)x+(1+α)uF′1(t)]∂∂u+αρF′1(t)∂∂ρ,V2=F2(t)∂∂x+F′2(t)∂∂u, V3=x∂∂x+u∂∂u,V4=x∂∂x+t∂∂t−ρ∂∂ρ, V5=∂∂x, V6=∂∂t, |
where V1 and V2 are the vector fields corresponding to the arbitrary functions F1(t) and F2(t) respectively.
The commutation relations of Lie algebra determined by Vi(i=1,2,⋯,6), which are shown as
[Vi,Vi]=0, i=1,2,⋯,6,[V1,V2]=−[V2,V1]=V6(−F′1F2−αF1F′2), [V1,V3]=−[V3,V1]=[V2,V5]=−[V5,V2]=0,[V3,V4]=−[V4,V3]=[V3,V6]=−[V6,V3]=[V5,V6]=−[V6,V5]=0,[V1,V4]=−[V4,V1]=V1(F1−tF′1), [V1,V5]=−[V5,V1]=V2(−F′1),[V1,V6]=−[V6,V1]=V1(−F′1), [V2,V3]=−[V3,V2]=V2(F2),[V2,V4]=−[V4,V2]=V2(F2−tF′2), [V2,V6]=−[V6,V2]=V2(−F′2),[V3,V5]=−[V5,V3]=−V5, [V4,V5]=−[V5,V4]=−V5, [V4,V6]=−[V6,V4]=−V6. |
It is obvious that the vector fields Vi(i=1,2,⋯,6) are closed under the Lie bracket.
In this section, we will get similarity variables and its symmetry reductions. By solving the reduced equations, some exact solutions of the system (1.3) will be presented.
Based on the infinitesimals (2.6), the similarity variables are found by solving the corresponding characteristic equations
dxξ=dtτ=duϕ=dρψ. |
Case 1 Let C1=C2=F1(t)=0, C3(≠0) and C4 be arbitrary constants, F2(t) is an arbitrary functions of t, then by solving the characteristic equation one can get the similarity variables
ω=x−∫F2(t)+C4C3dt, f(ω)=u−F2(t)C3, g(ω)=ρ, |
and the group-invariant solution is
{u=F2(t)C3+f(ω),ρ=g(ω). | (3.1) |
Substituting the group-invariant solution (3.1) into system (1.3), we reduce equation (1.3) to the following ODE:
{C4f‴−C3ff‴−(1−α)C3f′f″+C3κgg′=0,C4g′+αC3f′g−C3fg′=0, | (3.2) |
where f′=df/dω,g′=dg/dω.
Case 2 Let C1,C3 be arbitrary non-zero constants, C2=C4=F1(t)=F2(t)=0, then by solving the characteristic equation one can get the similarity variables
ω=xexp(−C1tC3), f(ω)=uexp(−C1tC3), g(ω)=ρ, |
and the group-invariant solution is
{u=exp(C1tC3)f(ω),ρ=g(ω). | (3.3) |
Substituting the group-invariant solution (3.3) into system (1.3), we reduce (1.3) to the following ODE:
{C1ωf‴−C3ff‴+C3(α−1)f′f″+C1f″+C3κgg′=0,C1ωg′+αC3f′g−C3fg′=0, | (3.4) |
where f′=df/dω,g′=dg/dω.
Case 3 Let F1(t)=kt,F2(t)=0, C1,C2,C3,C4 and k be constants which satisfy C2−αk≠0 and k+C1+C2≠0, then by solving the characteristic equation one can get the similarity variables
ω=[(k+C1+C2)x+C4](−αkt+C2t+C3)−k+C1+C2C2−αkk+C1+C2,f(ω)=u[(C2−αk)t+C3]−αk+C1+kC2−αk,g(ω)=ρ[(C2−αk)t+C3], |
and the group-invariant solution is
{u=[(C2−αk)t+C3]αk+C1+kC2−αkf(ω),ρ=g(ω)(C2−αk)t+C3. | (3.5) |
Substituting the group-invariant solution (3.5) into system (1.3), we reduce (1.3) to the following ODE:
{−(k+C1+C2)ωf‴+ff‴+(1−α)f′f″−κgg′=0,−(k+C1+C2)ωg′−αf′g+fg′=0, | (3.6) |
where f′=df/dω,g′=dg/dω.
In this section, we will derive the solutions of system (1.3) by using the symbolic computation [15,16,17]. Suppose that the solution of equation (3.2) is in the form
f=a0+a1F+a2F2,g=b0+b1F+b2F2 | (4.1) |
where F(ω) expresses the solution of the following generalized Riccati equation
F′=r+pF+qF2, | (4.2) |
and r,p,q are real constants. Substituting (4.1) along with (4.2) into (3.2) and collecting all terms with the same power in Fi(i=0,1,⋯,7) and setting the coefficients to zero yields a system of algebraic equations. Solving the algebraic equations and we can have the following results
α=2,a0=±√2κb2p4q2+C4C3,a1=±√2κb22q,a2=0,b0=b2p24q2,b1=b2pq, | (4.3) |
with b2,p,q,r,C3,C4 are constants and κ is a positive constant.
The solutions of equation (4.2) are listed as follows:
(a) When p2−4qr>0 and pq≠0 (qr≠0),
F1=−12q[p+√p2−4qrtanh(√p2−4qr2ω)],F2=−12q[p+√p2−4qrcoth(√p2−4qr2ω)],F3=−12q[p+√p2−4qr[tanh(√p2−4qrω)±isech(√p2−4qrω)]],F4=12q[−p+√p2−4qr[√A2+B2−Acosh(√p2−4qrω)]Asinh(√p2−4qrω)+B],F5=12q[−p−√p2−4qr[√B2−A2+Asinh(√p2−4qrω)]Acosh(√p2−4qrω)+B], B2−A2>0,F6=2rcosh(√p2−4qr2ω)√p2−4qrsinh(√p2−4qr2ω)−pcosh(√p2−4qr2ω),F7=2rsinh(√p2−4qr2ω)√p2−4qrcosh(√p2−4qr2ω)−psinh(√p2−4qr2ω), |
where A,B are arbitrary constants.
(b) When p2−4qr<0 and pq≠0 (qr≠0),
F8=12q[−p+√4qr−p2tan(√4qr−p22ω)],F9=−12q[p+√4qr−p2cot(√4qr−p22ω)],F10=12q[−p+√4qr−p2[tan(√4qr−p2ω)±sec(√4qr−p2ω)]],F11=12q[−p+√4qr−p2[√A2−B2−Acos(√4qr−p2ω)]Asin(√4qr−p2ω)+B], A2−B2>0,F12=12q[−p−√4qr−p2[√A2−B2−Asin(√4qr−p2ω)]Acos(√4qr−p2ω)+B], A2−B2>0,F13=−2rcos(√4qr−p22ω)√4qr−p2sin(√4qr−p22ω)+pcos(√4qr−p22ω), |
F14=2rsin(√4qr−p22ω)√4qr−p2cos(√4qr−p22ω)−psin(√4qr−p22ω), |
where A,B are arbitrary constants.
(c) When r=0 and pq≠0,
F15=−pCq[cosh(pω)−sinh(pω)+C],F16=−p[sinh(pω)+cosh(pω)]q[sinh(pω)+cosh(pω)+C], |
where C is an arbitrary constant.
(d) When p=r=0 and q≠0,
F17=−1qω+C, |
where C is an arbitrary constant.
Substituting (4.3) into (4.1) and (3.1), then we can obtain the following different exact solutions of system (1.3):
(a1) If Δ=p2−4qr>0 and pq≠0 (qr≠0), then the solutions of system (1.3) with α=2 can be derived as
{u1(x,t)=F2(t)+C4C3±√2κb2√Δ4q2tanh(√Δ2ω),ρ1(x,t)=b2Δ4q2tanh2(√Δ2ω), | (4.4) |
where ω=x−∫F2(t)C3dt.
If we take F(t)=F2(t)+C4C3,√Δ=2c1(c1>0),b=b24q2, then the above solution can be expressed as a simple form as
{u1(x,t)=F(t)±2√2κbc1tanh(c1ω),ρ1(x,t)=4bc21tanh2(c1ω), | (4.5) |
where ω=x−∫F(t)dt, and c1(>0),b,κ are constants.
Similarly, we can derive the other solutions of system (1.3) as
{u2(x,t)=F(t)±2√2κbc1coth(c1ω),ρ2(x,t)=4bc21coth2(c1ω). | (4.6) |
{u3(x,t)=F(t)±2√2κbc1[tanh(2c1ω)±isech(2c1ω)],ρ3(x,t)=4bc21[tanh(2c1ω)±isech(2c1ω)]2. | (4.7) |
{u4(x,t)=F(t)±2√2κbc1√A2+B2−Acosh(2c1ω)Asinh(2c1ω)+B,ρ4(x,t)=4bc21[√A2+B2−Acosh(2c1ω)Asinh(2c1ω)+B]2, | (4.8) |
where A,B are arbitrary constants.
{u5(x,t)=F(t)±2√2κbc1√B2−A2+Asinh(2c1ω)Acosh(2c1ω)+B,ρ5(x,t)=4bc21[√B2−A2+Asinh(2c1ω)Acosh(2c1ω)+B]2, | (4.9) |
where B2−A2>0.
{u6(x,t)=F(t)±2√2κbc1[psinh(c1ω)−2c1cosh(c1ω)2c1sinh(c1ω)−pcosh(c1ω)],ρ6(x,t)=4bc21[psinh(c1ω)−2c1cosh(c1ω)2c1sinh(c1ω)−pcosh(c1ω)]2. | (4.10) |
{u7(x,t)=F(t)±2√2κbc1[pcosh(c1ω)−2c1sinh(c1ω)2c1cosh(c1ω)−psinh(c1ω)],ρ7(x,t)=4bc21[pcosh(c1ω)−2c1sinh(c1ω)2c1cosh(c1ω)−psinh(c1ω)]2. | (4.11) |
(a2) When Δ=p2−4qr<0 and pq≠0 (qr≠0), if we denote F(t)=F2(t)+C4C3,√−Δ=2c1(c1>0),b=b24q2, then the solutions of system (1.3) with α=2 can be derived as
{u8(x,t)=F(t)±2√2κbc1tan(c1ω),ρ8(x,t)=4bc21tan2(c1ω). | (4.12) |
{u9(x,t)=F(t)±2√2κbc1cot(c1ω),ρ9(x,t)=4bc21cot2(c1ω). | (4.13) |
{u10(x,t)=F(t)±2√2κbc1[tan(2c1ω)±isech(2c1ω)],ρ10(x,t)=4bc21[tan(2c1ω)±isech(2c1ω)]2. | (4.14) |
{u11(x,t)=F(t)±2√2κbc1√A2−B2−Acos(2c1ω)Asin(2c1ω)+B,ρ11(x,t)=4bc21[√A2−B2−Acos(2c1ω)Asin(2c1ω)+B]2, | (4.15) |
where A,B are arbitrary constants and A2−B2>0.
{u12(x,t)=F(t)±2√2κbc1√A2−B2−Asin(2c1ω)Acos(2c1ω)+B,ρ12(x,t)=4bc21[√A2−B2−Asin(2c1ω)Acos(2c1ω)+B]2, | (4.16) |
where A2−B2>0.
{u13(x,t)=F(t)±2√2κbc1[psin(c1ω)−2c1cos(c1ω)2c1sin(c1ω)+pcos(c1ω)],ρ13(x,t)=4bc21[psin(c1ω)−2c1cos(c1ω)2c1sin(c1ω)+pcos(c1ω)]2. | (4.17) |
{u14(x,t)=F(t)±2√2κbc1[pcos(c1ω)+2c1sin(c1ω)2c1cos(c1ω)−psin(c1ω)],ρ14(x,t)=4bc21[pcos(c1ω)+2c1sin(c1ω)2c1cos(c1ω)−psin(c1ω)]2. | (4.18) |
(a3) When r=0 and pq≠0, if we denote F(t)=F2(t)+C4C3,b=b24q2, then the solutions of system (1.3) with α=2 can be derived as
{u15(x,t)=F(t)±√2κbp(1−2Ccosh(pω)−sinh(pω)+C),ρ15(x,t)=bp2(1−2Ccosh(pω)−sinh(pω)+C)2, | (4.19) |
where ω=x−∫F(t)dt, F(t) is an arbitrary function and b,C are constants.
{u16(x,t)=F(t)±√2κbp(1−2Csinh(pω)+cosh(pω)+C),ρ16(x,t)=bp2(1−2Csinh(pω)+cosh(pω)+C)2. | (4.20) |
(a4) When p=r=0 and q≠0, if we denote F(t)=F2(t)+C4C3,b=b24q2, then the solution of system (1.3) with α=2 can be derived as
{u17(x,t)=F(t)±2√2κb1ω+C,ρ17(x,t)=4b(1ω+C)2, | (4.21) |
where ω=x−∫F(t)dt, F(t) is an arbitrary function and b,C are constants.
In order to show the properties of the above solutions visually, we plot the 2D-graphs of some typical solutions. Some wave figures are given as follows (Figures 1–5):
For the solution (4.5), if we take the integration constant as 0 in ω=x−∫F(t)dt, then we plot the solution for the plus sign in u1 as
For the solution (4.6), if we take the integration constant as 0 in ω=x−∫F(t)dt, then we plot the solution for the plus sign in u2 as
For the solution (4.8), if we take the integration constant as 0 in ω=x−∫F(t)dt, then we plot the solution for the plus sign in u4 as
For the solution (4.10), if we take the integration constant as 0 in ω=x−∫F(t)dt, then we plot the solution for the plus sign in u6 as
For the solution (4.17), if we take the integration constant as 0 in ω=x−∫F(t)dt, then we plot the solution for the plus sign in u13 as
Remark 1 If we take F(t) as a constant, then all of the above solutions of system (1.3) are traveling wave solutions.
Remark 2 For the reduced equations (3.4) and (3.6), there exist a power series solutions [18,19]. We omit the details here for brevity.
In this section, we use the direct multiplier method [20] to derive a conservation law for system (1.3). The zero-order multipliers Λ1(t,x,u,ρ), Λ2(t,x,u,ρ) for the system (1.3) are determined by
{δδu[Λ1(uxxt+uuxxx+(1−α)uxuxx−κρρx)+Λ2(ρt+uρx−αuxρ)]=0δδρ[Λ1(uxxt+uuxxx+(1−α)uxuxx−κρρx)+Λ2(ρt+uρx−αuxρ)]=0, | (5.1) |
where δδu,δδρ are Euler-Lagrange operators defined by
δδu=∂∂u−Dx∂∂ux+D2x∂∂uxx−DtD2x∂∂uxxt−D3x∂∂uxxx,δδρ=∂∂ρ−Dt∂∂ρt−Dx∂∂ρx. | (5.2) |
Expanding (5.1) and splitting with respect to derivative of u,ρ, we obtain the following determining equations
Λ1u=0, Λ1ρ=0, Λ1x=0, Λ2u=0, Λ2t=0, Λ2x=0,αρΛ2ρ+uΛ2u+(1+α)Λ2=0. | (5.3) |
Then we obtain the solution
Λ1(t,x,u,ρ)=H(t), Λ2(t,x,u,ρ)=Aρ−1+αα, | (5.4) |
where A is an arbitrary constant, H(t) is an arbitrary functions with respect to t. From the solution (5.4), we can see that system (1.3) has one zero-order multiplier in the form of Λ1=H(t), Λ2=ρ−1+αα. So a conservation law of system (1.3) is
Dt(−αρ−1α)+Dx(H(t)uxt+H(t)uuxx−α2H(t)u2x−κ2H(t)ρ2−αuρ−1α)=0. | (5.5) |
In this paper, a generalized 2-HS system is investigated by using the classical Lie group method. First, Lie symmetry analysis was performed for the generalized 2-HS system, and its infinitesimal generator, geometric vector fields and commutation table of Lie algebra were obtained. Then, all of the similarity variables and its symmetry reductions of this equation are obtained. And by solving the reduced equations, some new exact solutions including traveling wave solutions of this generalized 2-HS system are constructed successfully. These are new solutions for the generalized 2-HS system. Finally, a conservation law of the generalized 2-HS system are shown by using the multiplier method.
This work is supported by the National Natural Science Foundation of China (No.11461022) and Applied Basic Research Foundation of Yunnan Province (Nos. 2018FH001-013 and 2018FH001-014), the Science Research Foundation of Yunnan Education Bureau (No. 2018JS479) and the Second Batch of Middle and Young Aged Academic Backbone of Honghe University (No. 2015GG0207).
The authors declare that there are no conflict interests regarding the publication of this paper.
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