# Step Soliton Generalized Solutions of the Shallow Water Equations

Authors: A. C. Alvarez; A. Meril; B. Valiño-Alonso
Journal: Journal of Applied Mathematics
 (2012)

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## Abstract

Generalized solutions of the shallow water equations are obtained.
One studies the particular case of a generalized soliton function passing by a variable bottom.
We consider a case of discontinuity in bottom depth. We assume that the surface elevation
is given by a step soliton which is defined using generalized solutions (Colombeau 1993).
Finally, a system of functional equations is obtained where the amplitudes and celerity
of wave are the unknown parameters. Numerical results are presented showing that the
generalized solution produces good results having physical sense.


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## Body

## 1. Introduction

The classical nonlinear shallow water equations were derived in [1]. There exist several works devoted to the applications, validations, or numerical solutions of these equations [2–5]. These equations provide a significant improvement over linear wave theory to describe the wave-breaking process [6].Shallow water equations have been submitted to numerous improvements to include several physical effects. In such sense, several dispersive extensions were developed. The inclusion of dispersive effects resulted in a big family of the so-called Boussinesq-type equations [7–10]. Many other families of dispersive wave equations have been proposed as well [11–13]. Other studies attempt to include the effect of different types of bottom shape [4, 14–19]. Also in [20, 21], the mild slope hypothesis is not required, and rapidly varying topographies was also considered. In these studies, the asymptotical expansion method was used. In [22] was included different geometry bathymetric by improving the shallow water equations by using variational principles.However, there are a few studies which attempt to include the discontinuous or not differentiable bottom effect into shallow water equations [23–25]. One reason is that in its deduction procedure, assume certain restrictions on bottom type function as differentiability. In [3], a numerical method to studding the discontinuous bottom was used.In this paper, we relaxedly completed this hypothesis allowing that the bottom function must be not differentiable by using the Colombeau algebra [26, 27] studying the shallow water equations with a discontinuous bottom. This algebra comes being used in several applications of the physics fields studying nonlinear partial differential equation. In this theory, the previous solutions are still valid because of the natural embedding of the distribution in the sense of Schwartz in this algebra. In particular the smooth functions are embedded as a constant sequence. However, this theory is specially useful when the product distribution is not allowed or when a formalism of continuous function is not more valid. Details of Colombeau algebra in the applications to hydrodynamics of can be found in [28].The method presented in this paper is general, and it can be used for a wide class of nonlinear dispersive wave equations such as Boussinesq-like system of equations. In order to try the possibilities of this theory, we consider the equation deduced in [6] with the principles that the equality p-po=ρg(ho+η) holds; here, p is the pressure, ho is the depth, ρ is the density of the water, and η is the surface elevation. This equality for the discontinuous bottom case is not more valid in the classical sense. So, we embedded the classical distribution in the generalized function where the nonlinear operations are allowed. Also, we consider the dispersive equations deduced in [8] which is valid to variable smooth bottom. Similar formulas obtained in this paper were obtained in [29] by using the method of the lines.To study the nonlinear and bottom irregularities effects, we consider the shallow water equations to simulate a generalized soliton passing by discontinuity in the bottom. The idea of taking a soliton to describe a traveling wave and singular solution as a soliton was developed by several works [30–35]. In [36], a generalized solution in the frame of Colombeau’s generalized functions was obtained. Solitons are used in coastal engineering to describe waves approximating to the coast with the presence of a vertical structure [37–41]. The evolution of a solitary wave at an abrupt junction was measured and discussed by [42] in detail. There exist a number of physical reasons to suppose that the propagation of a soliton wave over a discontinuity point in the bottom preserves the shape and the structure of an initial wave [43].The starting point, that the bottom has a discontinuity, constitutes a generalization of submerged structure or coral reef representation. This situation is equivalent, in practical engineering, to the presence of a vertical hard structure that in some cases breaks the wave propagation. As a wave propagates over the structure, part of the wave energy is reflected back to the open ocean, part of the energy is transmitted to the coast, and part of the energy is converted to turbulence and further dissipated in the vicinity of the structures [39, 44]. These processes we approximated by using two generalized solitons traveling in opposite direction.In this paper, we obtain generalized solutions of the shallow water equations in the one-dimensional case. The approximate solution is obtained as a singular solution. We suppose that in microscopic sense, when a wave crosses the discontinuity bottom point, one part continues its propagation to the shore, preserving the initial structure, while another part is reflected. We use a generalized soliton function which has macroscopic aspect in sense of Colombeau [27], that is, for a given τ1, Sτ1(τ)=0 for τ<-τ1, Sτ1(τ)=1 for -τ1<τ<τ1 and Sτ1(τ)=0 for τ>τ1. We obtain a nice procedure that reduces the problem of finding a solution of nonlinear partial differential equation to the one of solving a system of algebraic equations. Since this attempt used this theory to obtain practical formulas, we prove that in the limit, the Step generalized solution agreement reasonably with previous classical solutions. Moreover, we prove that by fixing some parameter that appears in this theory, some nonlinear and dispersive effects are reproduced well.This paper begins with a description of the Colombeau algebra. Some useful proposition including different product of generalized function was established to simplify some nonlinear operations. After that, generalized solutions are obtained for the flat bottom for two types of shallow water equations. In both cases the generalized solution is compared with previous formulas. Finally, we propose a method to obtain the generalized solution in the discontinuous bottom case. The accuracy of the numerical scheme for solving the shallow water equations was verified by comparing the numerical results with the theoretical solutions obtained by [45] and experimental data obtained in [46].


## 2. Colombeau Algebra

In this paper, we use a generalized solution deduced from the algebra of Colombeau [27, 47]. Such solution permits to construct a singular solution of the system of conservation law that preserves its structures and initial shape. These functions appear in the multiplication of distributions theory when nonlinear differential equations are studied.The mathematical theory of generalized solutions allows to obtain new formulas and numerical results [48]. The method proposed in [26, 49] is quite general, but each particular problem requires the definition of specific generalized functions. A general definition can be found in the specialized literature (see as an example [26, 27, 47]). Here, we present a version which is sufficient for the purpose of this paper. Let Ω be an open subset in ℝ. Putting
(2.1)Es(Ω)={R1:(ϵ,x)∈(0,1)×Ω⟶RsuchthatR1∈C∞(Ω),∀ϵ∈(0,1)},EM(Ω)={R1∈Es(Ω)/∀compactK⊂ΩandforalldifferentialoperatorD:∃q∈N,c>0,η>0suchthat|DR1(ϵ,x)|≤cϵ-q,∀x∈K,∀0<ϵ<η},N(Ω)={R1∈EM(Ω)/(∀K)⊂Ωcompactand∀Ddifferentialoperator,∃q∈N,∀p≥q,∃c>0,η>0,suchthat|DR1(ϵ,x)|≤cϵp-q,∀x∈K,∀0<ϵ<η},E
s
(
Ω
) and EM(Ω) are algebras, and N(Ω) is an ideal of Es(Ω).Definition 2.1.
The simplified algebra of generalized functions is the quotient spaceℑs(Ω)=Es(Ω)/N(Ω).The elementsG of ℑs(Ω) are denoted by G=R1(ϵ,x)+N(Ω). Distribution of compact support on ℝ can be embedded on ℑs(ℝ) by convolution with a mollifierρϵ, defined as follows: let ρ∈S(ℝ) (Schwartz’s space) with the properties ∫‍ρ(x)dx=1, ∫‍xαρ(x)dx=0, for all α∈N2,|α|>1, then we set ρϵ(x):=(1/ϵ)2ρ(x/ϵ). Then the generalized function ∫‍xαρɛ(x-y)w(x)dx+N(Ω) belongs to ℑs(ℝ) [28].ℑ
s
(
Ω
) is clearly an algebra with the usual pointwise operations of addition, inner multiplication, and exterior multiplication by scalars. In this algebra, there are two equalities, one strong (=) and one weak (~). The strong one is the classical algebraic equality. The weak one is called association and is denoted by the symbol ~; in other words, two simplified generalized functions are equal if the difference of two of their representatives belongs to the ideal N(Ω). Also, whereas multiplication is compatible with equality in ℑs(Ω), it is not compatible with association. Therefore, the distinction between (=) and (~) automatically ensures that the physically correct solution is selected, a distinction that can be made in analytical as well as in numerical calculations by using a suitable algorithm [27, 28].Definition 2.2.
Two generalized functionsG1,G2∈ℑs(Ω) are associated, G1~G2, if there exists representatives R1,R2∈Es(Ω) of G1, G2 respectively, such that: for all ψ∈D(ℝ),   ∫ℝ‍(R1(ϵ,x)-R2(ϵ,x))ψ(x)dx→0whenϵ→0.In the interpretation of the generalized solution, we use that two different generalized functions associated with the same distribution differ by an infinitesimal.It is well known from the classical asymptotical method that the several solutions depend on an infinitesimalϵ. For example, in [6, page 470], the solution of the Korteweg de Vries is given in linear limit as ςϵ=λcos(ϵ(x-ct)), whereas in the solitary waves limit as ςϵ=λsech(ϵ(x-ct)). In [36], similar solutions are obtained in the sense of Colombeau. These functions show that even in the classical sense, the solution is given by a family of functions. The idea to look for a generalized solution in the sense of Colombeau means to seek a solution like a family that depend of one infinitesimal, but this extension must guarantee that they keep valid the association by differentiation and nonlinear operations between them.The generalized functions have useful properties for our purpose:(i)
C∞(Ω)⊂ℑs(Ω),(ii)
letρ∈D(ℝ) be a C∞(ℝ) function such that ∫ℝ‍ρ(x)dx=1. Then the class of R1(ϵ,x)=(1/ϵ)ρ(x/ϵ) is an element of ℑs(Ω) associated with the Dirac delta function, that is, for all ψ∈D(ℝ), ∫ℝ‍R1(ϵ,x)ψ(x)dx→ψ(0), when ϵ→0, where D(ℝ) denotes the space of the infinitely smooth functions on ℝ with compact support.(iii)
it is possible to define the integral of generalized functions in the following way: letG∈ℑs(ℝ) and R1∈Es(ℝ) a representative. The application R2:(ϵ,x)∈(0,1)×ℝ→ℝ is defined by
(2.2)(ϵ,x)⟶R2(ϵ,x)=∫xox‍R1(ϵ,x)dx,then R2∈Es(ℝ), for all xo∈ℝ. The class J∈ℑs(ℝ) of R2 verifies dJ/dx=J′=G and is called a primitive of G.The association~ is stable by differentiation but not by multiplication, that is, if G1,G2,G∈ℑs(ℝ), and G1~G2 then G1′~G2′, but GG1 and GG2 are not necessarily associated.Definition 2.3.
A generalized functionH∈ℑs(ℝ) is called a Heaviside generalized function if it has representative R∈Es(ℝ) such that there exists a sequence of real numbers A(ϵ)>0, A(ϵ)→0, when ϵ→0 such that(i)
R(ϵ,x)=0, for all ϵ>0, and x<-A(ϵ),(ii)
R(ϵ,x)=1, for all ϵ>0, and x>A(ϵ),(iii)
sup|R(ϵ,x)|<+∞, ϵ>0, and x∈ℝ.The Heaviside generalized functions are associated between them. Moreover,Hn~H for n∈ℕ, n>0.Definition 2.4.
A generalized functionδ∈ℑs(ℝ) is called Dirac generalized function if it has a representative R∈Es(ℝ) such that there exists a sequence A(ϵ)>0, A(ϵ)→0, when ϵ→0 such that(i)
R(ϵ,x)=0, for all ϵ>0, and |x|>A(ϵ),(ii)
∫ℝ‍R(ϵ,x)dx=1, for all ϵ>0,(iii)
∫ℝ‍|R(ϵ,x)|dx<C, for all ϵ>0, where C is a constant independent of ϵ.It is possible to check that the relationH′~δ holds between Heaviside and Dirac generalized functions. Moreover, for a reasonable Heaviside and Dirac generalized function, there exists a constant M such that Hδ~Mδ.Definition 2.5.
For a givenτ1>0, a generalized function Sτ1∈ℑs(ℝ) is called a step soliton generalized function if it has a representative R∈Es(ℝ) defined by(i)
R(ϵ,x)=R1(ϵ,x-τ1)-R2(ϵ,x+τ1),where R1,R2∈Es(ℝ) are representative, of a Heaviside generalized function.For instance,R1(ϵ,x)=0 if x+τ1≤0, R1(ϵ,x)=1 if x+τ1≥ɛ, and R1(ϵ,x)>0 if 0<x+τ1ɛ (see Figure 1(a)). Besides, R1(ϵ,x)=0 if x-τ1≤0, R1(ϵ,x)=1 if x-τ1≥ɛ, and R1(ϵ,x)>0 if 0<x-τ1ɛ (see Figure 1(b)). In Figure 1(c), the graph of R1(ϵ,x+τ1)-R1(ϵ,x-τ1) is shown.Sketch of a representative of step soliton generalized function.
(a)
(b)
(c)From Definition2.5, we obtain that the equality Sτ1(x)=H(x+τ1)-H(x-τ1) holds. Moreover, the macroscopic aspect of the step generalized function is not necessarily symmetric (see Figure 1). A lesson from this application is that by assuming that physically relevant distributions such as Heaviside H and Dirac δ generalized function are elements of ℑs(ℝ); one gets a picture that is much closer to reality than if they are restricted to classical sense. This fact can be exploited in mathematical and physical modeling. We can verify that the step generalized soliton has one as the maximum value of its representatives. Thus, it is possible to verify that the generalized function λSτ1 has λ as the maximum values.Definition 2.6.
A generalized functionδ1∈ℑs(ℝ) is called a microscopic soliton generalized function if it has a representative R∈Es(ℝ) defined by(i)
R(ϵ,x)=1-R1(ϵ,x)-R1(ϵ,-x),where R1∈Es(ℝ) is a representative of a Heaviside generalized function.From Definition2.6, we obtain that the relation δ1(τ)=(1-H(τ)-H(-τ)) holds. Moreover, δ1 generates a family of generalized functions with different height γ, that is, δγ(τ)=γδ1(τ). Let us denote by θ the function that satisfies
(2.3)θ(x)=0,forx<0,θ(x)=π2,forx=0,θ(x)=0,forx>0.
Then the function θ has the macroscopic aspect of the generalized function δπ/2=(π/2)δ1. Then we have
(2.4)δπ/2=θ,
where θ is given in (2.3), and δπ/2 is the microscopic soliton with height π/2. Let us define the composite function
(2.5)cos⁡(θ(x))=0,forx<0,cos⁡(θ(x))=π2,forx=0,cos⁡(θ(x))=0,forx>0,
where θ(x) is given in (2.3). It is possible to check that the generalized function cos(θ(x)) has the macroscopic aspect of the generalized function 1-δ1, where δ1 is the microscopic soliton of height one, that is,
(2.6)cos⁡(δπ/2)=1-δ1.
Let us denote
(2.7)ϑ(x)=ϑ1,forx<0,ϑ(x)=ϑ2,forx>0,
with real numbers ϑ1>ϑ2. Now, using the Heaviside generalized function H, we can write
(2.8)ϑ(x)=ϑ1+(ϑ2-ϑ1)H(x).
We can check that the angle θ in respect of axis OX in each point of the function ϑ(x) is given by (2.3). Since tan(θ(x))=ϑ′(x), where ϑ′(x) is the derivative of ϑ(x), we have using (2.4) that
(2.9)tan(δπ/2)=(ϑ2-ϑ1)δ(x),
where δ is the Dirac generalized function.


## 3. Some Useful Lemmas

Reviewing cases of the product of two step generalized functions, the product with function Heaviside generalized function, and the product derivatives of step generalized functions, as well as products with the microscopic generalized functions, it should be noted that the depth with a discontinuity is closer to the combination of the Heaviside generalized functions. In the calculations with generalized function on the shallow water equations arise the derivatives of Heaviside generalized functions which are reasonably approximated by delta generalized function. In short, in the upcoming paragraph, we show those useful lemmas of the product of generalized functions that allow to simplify the calculations and obtain in this way algebraic equations.To prove the main results of this paper these lemmas of generalized functions are needed. Such lemmas consist in simplifing association between the product of several generalized functions that appears in the algebras of substitution of the proposal solution in the shallow water equations. Let us prove the following.Lemma 3.1.
Givenτ1>0, let it be denoted by Sτ1 and H the step and Heaviside generalized functions respectively. Then the following relations hold:
(3.1)Sτ1′(x-ct)H(x)~MSτ1′(x-ct),(3.2)Sτ1′(x+ct)H(x)~0,
where M, c>0 are constants and t>0.Proof.
We have thatSτ1′(x-ct)=δ(x-ct+τ1)-δ(x-ct-τ1). From this there exists constant M such that for t>0, c>0, and ct-τ1>0, we have δ(x-ct+τ1)H(x)~Mδ(x-ct+τ1) and δ(x-ct-τ1)H(x)~Mδ(x-ct-τ1), then (3.1) holds.
It possible to check that fort>0, c>0, and -ct+τ1<0, (3.2) holds.Lemma 3.2.
Givenτ1>0, let it be denoted by Sτ1 the step generalized functions. Then the following relations hold:
(3.3)Sτ1(x-ct)δ(x)~0,(3.4)Sτ1(x+ct)δ(x)~0,
for t>0 and c>0.Proof.
We have thatSτ1(x-ct)=H(x-ct+τ1)-H(x-ct-τ1), δ(x)H(x-ct+τ1)~0, and δ(x)H(x-ct+τ1)~0 for t>0 and c>0; thus, (3.3) holds. Analogously, it is possible to verify that (3.4) holds.The following propositions are useful.Lemma 3.3.
Givenτ1>0, c>0, and t such that t>τ1/c, let it be denoted by Sτ1 and Sτ1′ the step soliton and its derivative generalized functions, respectively. Then the following relations hold:(i)
Sτ12~Sτ1,(ii)
Sτ1(x-ct)Sτ1′(x+ct)~0,(iii)
Sτ1′(x-ct)Sτ1(x+ct)~0.Proof.
We prove here that (ii) the others are similar. We have thatSτ1(x-ct)=H(x-ct+τ1)-H(x-ct-τ1) and Sτ1′(x+ct)=δ(x+ct+τ1)-δ(x+ct-τ1), where δ and H are the Dirac and Heaviside generalized function. It is possible to check that for t>τ1/c, the delta soliton of the Sτ1′(x-ct) stays in the null part of step soliton Sτ1(x-ct), so (ii) holds.Lemma 3.4.
Givenτ1>0, c>0, and t such that t>τ1/c, let it be denoted by Sτ1 and δ1 the step soliton and microscopic generalized functions, respectively. Then the following relations hold:(i)
Sτ1′(x+ct)δ1(x)~0,(ii)
Sτ1′(x-ct)δ1(x)~0.


## 4. The Flat Bottom Case

### 4.1. Nonlinear Effect

We consider the so-called shallow water equations in one dimension as given in [6]. Here, we put these equations in the sense of associations of Colombeau as follows:
(4.1)ht+(hu)x~0,(4.2)(u)t+12(u2)x+ghx~0,
where h is the height of water, u is the velocity, and g is the gravity constant. This model is relevant even to deep water as long as the velocity stays constant on the thickness of the water layer, otherwise this model corresponds to a damped model since the velocity is averaged which can be deduced, as seen easily; by using the Cauchy Schwartz inequality. We split the height of water as h=ho+η, where ho is the bottom depth, and η is the surface elevation relative to the fixed depth ho (which is the case in Figure 2 if the angle in respect to the OX axis is zero, i.e., θ=0). As in [24], we take the following.Figure 2
Schematic diagram of a solitary wave propagating over a mild slope bottom.Assumption 4.1.
Particles in a vertical plane at any instant always remain in a vertical plane, that is, the streamwise velocity is uniform over the vertical. Each vertical plane always contains the same particles; hence, the integration volume is moving with the fluid.With the previous assumption, we have chosen a material reference frame to describe the motion of the soliton in the fluid.For a givenτ1, let us denote by Sτ1′ the derivative of the step soliton generalized function Sτ1. We interpret (4.1) and (4.2) in the sense of association, that is, we seek the analog of classical weak solutions (see [26, 27, 47, 50]). We are going to seek solutions of the system (4.1) and (4.2) in the form of λSτ1 where Sτ1 is a step soliton generalized function. The following theorem holds.Theorem 4.2.
It is assumed that solitons of the system (4.1) and (4.2) are given by(4.3a)η=λSτ1(x-X(t)),(4.3b)u=uoSτ1(x-X(t)),for a given τ1, where λ and uo are constants representing the amplitude of surface elevation and particle velocity, respectively, and h=ho+η, where ho is a fixed real number. Here, X(t) is the trajectory where the singularity travels and c=X′(t) denotes the soliton velocity. Assuming that λ is known, then the wave velocity c and amplitude of particle velocity α are given by(4.4a)uo=λgho+λ/2,(4.4b)c=(ho+λ)gho+λ/2.Proof.
Using thath=ho+η and substituting (4.3a) and (4.3b) in (4.1) with ξ=x-X(t), we obtain
(4.5)λ(-X′)Sτ1′(ξ)+uoλSτ1(ξ)Sτ1′(ξ)+uoλSτ1(ξ)Sτ1′(ξ)+houoSτ1′(ξ)~0.
Now, using that Sτ1(ξ)Sτ1′(ξ)=(1/2)(Sτ12(ξ))′, we have
(4.6)λ(-X′)Sτ1′(ξ)+uoλ(Sτ12(ξ))′+houoSτ1′(ξ)~0.
Finally, from the fact that Sτ12(ξ)~Sτ1(ξ), we deduce that
(4.7)λ(-X′)Sτ1′(ξ)+uoλSτ1′(ξ)+houoSτ1′(ξ)~0.
Since Sτ1′(ξ) is not associate to null generalized function, such above equation implies that(4.8a)-X′λ+uoλ+houo=0,(4.8b)X′=uo(λ+ho)λ.Since that right hide side of (4.8b) is a constant, then the trajectory of the singularity is the straight line rect, that is,
(4.9)X′(t)=uo(λ+ho)λt+K,
where K is a constant. As a consequence, the soliton velocity is given by
(4.10)c=X′(t)=uo(λ+ho)λ.
Now, substituting (4.3a) and (4.3b) in (4.2) and using again the fact that Sτ1Sτ1′=(1/2)(Sτ12)′, we obtain
(4.11)uo(-X′)Sτ1′+12uo2(Sτ12)′+gλSτ1′~0,
or equivalently,
(4.12)(-X′uo+uo22+gλ)Sτ1′~0.
Since Sτ1′ is not associate to null generalized function, from (4.12), we obtain
(4.13)-X′uo+uo22+gλ=0.
Substituting (4.10) in (4.13), we have
(4.14)-2uo2(ho+λ)+2gλ2+λuo2=0.
From (4.14) we obtain (4.4a), and from (4.4a) and (4.10) we obtain that (4.4b) holds.Remark 4.3.
The choice of the particle velocityu as a product by the step generalized function (see (4.3b)) like the free surface stays in concordance which linear wave theory, see as an example [45, 51].Remark 4.4.
Taking off the amplitude waveλ from (4.4b) and substituting in (4.4a) we obtain
(4.15)uo=uohoc-uogho+(uoho/(c-uo)).
Thus, we obtain a close system of equations with (4.4a) and (4.4b), and (4.15), which allows to estimate the wave celerity, velocity particle, and wave amplitude (c,uo,λ) by using quasi-Newton method, for example.Theorem4.2 has an immediate practical sense: the trajectory of the singularity is linear for the case of planar bottom with the system of (4.1) and (4.2).Let us denoteσ=λ/ho, μ=(hk)2, where k is number wave, as the nonlinear and dispersive parameters, respectively. From now, we compared the formulas obtained with previous solutions. To do so, we compared the wave celerity of different formulations (see [52]). It is possible to rewrite the wave celerity (4.4b) as follows:
(4.16)c=gho1+λ/ho1+λ/2ho11+λ/2ho.
Equation (4.16) for small nonlinear parameter σ≪1 holds,
(4.17)c=gho(1+34λho-532(λho)2+7128(λho)3+O(λho)4).
Formula (4.17) is similar to those obtained in [6, 53–55] which depends on the nonlinear parameter σ. It is possible to check that the difference of the formula  (4.4b) in respect of those obtained in the above-cited review has order σ. In particular, we consider the wave celerity obtained in ([6, page 463]), that is, c1=(3g(ho+λ)-2gho)=gho(3(1+λ/ho)1/2-2), which for small σ holds as follow,
(4.18)c1=gho(1+32λho-38(λho)2+316(λho)3+O(λho)4).
It is possible to verify that the quotient between (4.17) and (4.18) is approximately |c|/|c1|≈1-(3/4)σ+(43/32)σ2+(311/128)σ3. Thus, we obtain good matches (maximum difference of less than 10 percent) for σ<0.4 (see Figure 3(a)).Quotient of wave celerity for two formulations. In the case (a), only nonlinear effect was simulated. In the case (b), the dispersive and nonlinear have the same orderσ=O(μ).
(a)
Nonlinear effect
(b)
Nonlinear and dispersive of the same orderσ=O(μ)Also, whenσ=O(μ), the formula for the wave celerity (4.17) is similar to those obtained in [8, 25, 56, 57]. In particular, the quotient in respect to the classical dispersion linear (Airy’s wave celerity):
(4.19)c2=ghotanh(kh)kh=gho(1-16(kh)2+19360(kh)4-553024(kh)6+O((kh)8))
is approximately |c|/|c1|≈1+(11/12)μ-(9/160)μ2-(53/17280)μ3. Thus, we obtain maximum difference of less than 10 percent for μ<0.1 (see Figure 3(b)). This small range of good matches is expected because in the deduction of (4.4a) and (4.4b), we do not consider the dispersive effect in shallow water equations.


### 4.2. Nonlinear and Dispersive Effects

We consider the following so-called shallow water equations with dispersive effect in one dimension as given in [8]:
(4.20)ηt+hux+(ηu)x+(α+13)h3uxxx=0,(u)t+gηx+12(u2)x+αh2utxx=0,
where h is the height of water, u is the velocity, g is the gravity constant, and α=(1/2)(zα/h)2+(zα/h) at reference depth zα. We assume here that the bottom is constant, that is, h=ho. But with the method presented in this paper, it is possible to obtain generalized solutions regarding variable bottom.The following theorem holds.Theorem 4.5.
It is assumed that solitons of the system (4.20) are given by
(4.21)η=λSτ1(kx-ωt),u=uoSτ1(kx-ωt),
for a given τ1, where λ and uo are constants representing the amplitude of surface elevation and particle velocity, respectively, and h=ho+η, where ho is a fixed real number. Here, k,ω are the wave number and frequency, respectively. Then the following equalities hold:
(4.22)uo=λghoho1(1+σ/2)+(ν2/2)αμ((1+σ)+ν1(α+(1/3)μk)),(4.23)ω=uokλ(λ+ho+ν1(α+13)μho),
where ν1, ν2 are arbitrary constants and σ and μ are the nonlinear and dispersive parameters, respectively.Proof.
Since the proof is similar to Theorem4.2, we present a summary here. The idea of the proof consists in substituting the generalized function (4.21) in the system (4.20). By using the relations Sτ12(ξ)~Sτ1(ξ) and Sτ1(ξ)Sτ1′(ξ)=(1/2)(Sτ12(ξ))′, ξ=kx-ωt and after several operations, we obtain
(4.24)(-ωλ+uok(ho+λ))Sτ1′(ξ)+(α+13)k3ho3uoSτ1′′′(ξ)~0,(-uoω+12uo2k+gλk)Sτ1(ξ)-αk2ho2uoωSτ1′′′(ξ)~0.
Finally, taking a representant R(ϵ,ξ)=a1+a2ϵξ+a3ϵ2ξ2+a4ϵ3ξ3+O(ϵ4ξ4) of Sτ1 and using the Definition 2.2, we obtain that there exist constants ν1,ν2 such that
(4.25)ω=uok(ho+λ)λ+ν1(α+(1/3))k3uoho3λ,(4.26)-uoω+12uo2k+gλk-ν2αk2ho2ωuo=0.
Combining (4.25) and (4.26), we obtain (4.22) and (4.23).Remark 4.6.
Takingν1=ν2=0 in (4.25) and (4.26), that is, neglecting the dispersive effects, it is possible to verify that (4.22) and (4.23) are the same as that (4.4a) and (4.4b) in Theorem 4.2 (the nonlinear effect alone), which indicates that the calculations are consistent.From (4.23), we can deduce the wave celerity as
(4.27)c=gho(1+σ+ν1(α+(1/3))μ)(1+σ/2)+(1/2)ν2αμ((1+σ)+ν1(α+(1/3))μμ).
The expression (4.27) is similar to those obtained in [29]. In the following, we verify the similitude of formula (4.27) with Airy’s wave celerity. In the simulation we assume that σ=O(μ) and ho=1. Also we take the value of parameter α=-0.39 from [8]. In Figures 4(a) and 4(b), we present the quotient of the wave celerity (4.27) with Airy’s wave celerity, depending on the dispersive parameter μ from shallow water (0<μ<π/10) to transitional (π/10<μ<π). An optimum value of the parameter (ν1,ν2)=(4.17,-1.7) for the range, 0<μ<2.5 with σ=μ, by minimizing the sum of the relative difference between the two wave celerity studies was obtained here. We can see that several pairs of optimum parameters (ν1,ν2) produce good matches with greater interval which is better than the nonlinear case (see Figures 4(a) and 4(b)).Comparison of wave celerity for dispersive and nonlinear of the same orderσ=O(μ).
(a)
(b)


## 4.1. Nonlinear Effect

We consider the so-called shallow water equations in one dimension as given in [6]. Here, we put these equations in the sense of associations of Colombeau as follows:
(4.1)ht+(hu)x~0,(4.2)(u)t+12(u2)x+ghx~0,
where h is the height of water, u is the velocity, and g is the gravity constant. This model is relevant even to deep water as long as the velocity stays constant on the thickness of the water layer, otherwise this model corresponds to a damped model since the velocity is averaged which can be deduced, as seen easily; by using the Cauchy Schwartz inequality. We split the height of water as h=ho+η, where ho is the bottom depth, and η is the surface elevation relative to the fixed depth ho (which is the case in Figure 2 if the angle in respect to the OX axis is zero, i.e., θ=0). As in [24], we take the following.Figure 2
Schematic diagram of a solitary wave propagating over a mild slope bottom.Assumption 4.1.
Particles in a vertical plane at any instant always remain in a vertical plane, that is, the streamwise velocity is uniform over the vertical. Each vertical plane always contains the same particles; hence, the integration volume is moving with the fluid.With the previous assumption, we have chosen a material reference frame to describe the motion of the soliton in the fluid.For a givenτ1, let us denote by Sτ1′ the derivative of the step soliton generalized function Sτ1. We interpret (4.1) and (4.2) in the sense of association, that is, we seek the analog of classical weak solutions (see [26, 27, 47, 50]). We are going to seek solutions of the system (4.1) and (4.2) in the form of λSτ1 where Sτ1 is a step soliton generalized function. The following theorem holds.Theorem 4.2.
It is assumed that solitons of the system (4.1) and (4.2) are given by(4.3a)η=λSτ1(x-X(t)),(4.3b)u=uoSτ1(x-X(t)),for a given τ1, where λ and uo are constants representing the amplitude of surface elevation and particle velocity, respectively, and h=ho+η, where ho is a fixed real number. Here, X(t) is the trajectory where the singularity travels and c=X′(t) denotes the soliton velocity. Assuming that λ is known, then the wave velocity c and amplitude of particle velocity α are given by(4.4a)uo=λgho+λ/2,(4.4b)c=(ho+λ)gho+λ/2.Proof.
Using thath=ho+η and substituting (4.3a) and (4.3b) in (4.1) with ξ=x-X(t), we obtain
(4.5)λ(-X′)Sτ1′(ξ)+uoλSτ1(ξ)Sτ1′(ξ)+uoλSτ1(ξ)Sτ1′(ξ)+houoSτ1′(ξ)~0.
Now, using that Sτ1(ξ)Sτ1′(ξ)=(1/2)(Sτ12(ξ))′, we have
(4.6)λ(-X′)Sτ1′(ξ)+uoλ(Sτ12(ξ))′+houoSτ1′(ξ)~0.
Finally, from the fact that Sτ12(ξ)~Sτ1(ξ), we deduce that
(4.7)λ(-X′)Sτ1′(ξ)+uoλSτ1′(ξ)+houoSτ1′(ξ)~0.
Since Sτ1′(ξ) is not associate to null generalized function, such above equation implies that(4.8a)-X′λ+uoλ+houo=0,(4.8b)X′=uo(λ+ho)λ.Since that right hide side of (4.8b) is a constant, then the trajectory of the singularity is the straight line rect, that is,
(4.9)X′(t)=uo(λ+ho)λt+K,
where K is a constant. As a consequence, the soliton velocity is given by
(4.10)c=X′(t)=uo(λ+ho)λ.
Now, substituting (4.3a) and (4.3b) in (4.2) and using again the fact that Sτ1Sτ1′=(1/2)(Sτ12)′, we obtain
(4.11)uo(-X′)Sτ1′+12uo2(Sτ12)′+gλSτ1′~0,
or equivalently,
(4.12)(-X′uo+uo22+gλ)Sτ1′~0.
Since Sτ1′ is not associate to null generalized function, from (4.12), we obtain
(4.13)-X′uo+uo22+gλ=0.
Substituting (4.10) in (4.13), we have
(4.14)-2uo2(ho+λ)+2gλ2+λuo2=0.
From (4.14) we obtain (4.4a), and from (4.4a) and (4.10) we obtain that (4.4b) holds.Remark 4.3.
The choice of the particle velocityu as a product by the step generalized function (see (4.3b)) like the free surface stays in concordance which linear wave theory, see as an example [45, 51].Remark 4.4.
Taking off the amplitude waveλ from (4.4b) and substituting in (4.4a) we obtain
(4.15)uo=uohoc-uogho+(uoho/(c-uo)).
Thus, we obtain a close system of equations with (4.4a) and (4.4b), and (4.15), which allows to estimate the wave celerity, velocity particle, and wave amplitude (c,uo,λ) by using quasi-Newton method, for example.Theorem4.2 has an immediate practical sense: the trajectory of the singularity is linear for the case of planar bottom with the system of (4.1) and (4.2).Let us denoteσ=λ/ho, μ=(hk)2, where k is number wave, as the nonlinear and dispersive parameters, respectively. From now, we compared the formulas obtained with previous solutions. To do so, we compared the wave celerity of different formulations (see [52]). It is possible to rewrite the wave celerity (4.4b) as follows:
(4.16)c=gho1+λ/ho1+λ/2ho11+λ/2ho.
Equation (4.16) for small nonlinear parameter σ≪1 holds,
(4.17)c=gho(1+34λho-532(λho)2+7128(λho)3+O(λho)4).
Formula (4.17) is similar to those obtained in [6, 53–55] which depends on the nonlinear parameter σ. It is possible to check that the difference of the formula  (4.4b) in respect of those obtained in the above-cited review has order σ. In particular, we consider the wave celerity obtained in ([6, page 463]), that is, c1=(3g(ho+λ)-2gho)=gho(3(1+λ/ho)1/2-2), which for small σ holds as follow,
(4.18)c1=gho(1+32λho-38(λho)2+316(λho)3+O(λho)4).
It is possible to verify that the quotient between (4.17) and (4.18) is approximately |c|/|c1|≈1-(3/4)σ+(43/32)σ2+(311/128)σ3. Thus, we obtain good matches (maximum difference of less than 10 percent) for σ<0.4 (see Figure 3(a)).Quotient of wave celerity for two formulations. In the case (a), only nonlinear effect was simulated. In the case (b), the dispersive and nonlinear have the same orderσ=O(μ).
(a)
Nonlinear effect
(b)
Nonlinear and dispersive of the same orderσ=O(μ)Also, whenσ=O(μ), the formula for the wave celerity (4.17) is similar to those obtained in [8, 25, 56, 57]. In particular, the quotient in respect to the classical dispersion linear (Airy’s wave celerity):
(4.19)c2=ghotanh(kh)kh=gho(1-16(kh)2+19360(kh)4-553024(kh)6+O((kh)8))
is approximately |c|/|c1|≈1+(11/12)μ-(9/160)μ2-(53/17280)μ3. Thus, we obtain maximum difference of less than 10 percent for μ<0.1 (see Figure 3(b)). This small range of good matches is expected because in the deduction of (4.4a) and (4.4b), we do not consider the dispersive effect in shallow water equations.


## 4.2. Nonlinear and Dispersive Effects

We consider the following so-called shallow water equations with dispersive effect in one dimension as given in [8]:
(4.20)ηt+hux+(ηu)x+(α+13)h3uxxx=0,(u)t+gηx+12(u2)x+αh2utxx=0,
where h is the height of water, u is the velocity, g is the gravity constant, and α=(1/2)(zα/h)2+(zα/h) at reference depth zα. We assume here that the bottom is constant, that is, h=ho. But with the method presented in this paper, it is possible to obtain generalized solutions regarding variable bottom.The following theorem holds.Theorem 4.5.
It is assumed that solitons of the system (4.20) are given by
(4.21)η=λSτ1(kx-ωt),u=uoSτ1(kx-ωt),
for a given τ1, where λ and uo are constants representing the amplitude of surface elevation and particle velocity, respectively, and h=ho+η, where ho is a fixed real number. Here, k,ω are the wave number and frequency, respectively. Then the following equalities hold:
(4.22)uo=λghoho1(1+σ/2)+(ν2/2)αμ((1+σ)+ν1(α+(1/3)μk)),(4.23)ω=uokλ(λ+ho+ν1(α+13)μho),
where ν1, ν2 are arbitrary constants and σ and μ are the nonlinear and dispersive parameters, respectively.Proof.
Since the proof is similar to Theorem4.2, we present a summary here. The idea of the proof consists in substituting the generalized function (4.21) in the system (4.20). By using the relations Sτ12(ξ)~Sτ1(ξ) and Sτ1(ξ)Sτ1′(ξ)=(1/2)(Sτ12(ξ))′, ξ=kx-ωt and after several operations, we obtain
(4.24)(-ωλ+uok(ho+λ))Sτ1′(ξ)+(α+13)k3ho3uoSτ1′′′(ξ)~0,(-uoω+12uo2k+gλk)Sτ1(ξ)-αk2ho2uoωSτ1′′′(ξ)~0.
Finally, taking a representant R(ϵ,ξ)=a1+a2ϵξ+a3ϵ2ξ2+a4ϵ3ξ3+O(ϵ4ξ4) of Sτ1 and using the Definition 2.2, we obtain that there exist constants ν1,ν2 such that
(4.25)ω=uok(ho+λ)λ+ν1(α+(1/3))k3uoho3λ,(4.26)-uoω+12uo2k+gλk-ν2αk2ho2ωuo=0.
Combining (4.25) and (4.26), we obtain (4.22) and (4.23).Remark 4.6.
Takingν1=ν2=0 in (4.25) and (4.26), that is, neglecting the dispersive effects, it is possible to verify that (4.22) and (4.23) are the same as that (4.4a) and (4.4b) in Theorem 4.2 (the nonlinear effect alone), which indicates that the calculations are consistent.From (4.23), we can deduce the wave celerity as
(4.27)c=gho(1+σ+ν1(α+(1/3))μ)(1+σ/2)+(1/2)ν2αμ((1+σ)+ν1(α+(1/3))μμ).
The expression (4.27) is similar to those obtained in [29]. In the following, we verify the similitude of formula (4.27) with Airy’s wave celerity. In the simulation we assume that σ=O(μ) and ho=1. Also we take the value of parameter α=-0.39 from [8]. In Figures 4(a) and 4(b), we present the quotient of the wave celerity (4.27) with Airy’s wave celerity, depending on the dispersive parameter μ from shallow water (0<μ<π/10) to transitional (π/10<μ<π). An optimum value of the parameter (ν1,ν2)=(4.17,-1.7) for the range, 0<μ<2.5 with σ=μ, by minimizing the sum of the relative difference between the two wave celerity studies was obtained here. We can see that several pairs of optimum parameters (ν1,ν2) produce good matches with greater interval which is better than the nonlinear case (see Figures 4(a) and 4(b)).Comparison of wave celerity for dispersive and nonlinear of the same orderσ=O(μ).
(a)
(b)


## 5. A Discontinuity Bottom Case

In this section, we studied the case in which a soliton crosses a bottom discontinuity (see Figure5). Seeking the solution of shallow water equation requires some useful lemmas that were proved in Section 3. These propositions contain the key results of the product of generalized functions that appear in the algebraic operations when generalized solution is searched.Figure 5
Schematic diagram of a solitary wave propagating over a discontinuity bottom.


### 5.1. Generalized Solution

Following the same idea as in the previous section, we obtain a generalized solution of shallow water equation stated in [6] as in this case one takes into account friction and slope of the bottom
(5.1)ht+(hu)x=0,(5.2)(u)t+12(u2)x+g′hx=g′S-Cfu2,
where g′=gcos(θ), S=tan(θ) with bottom slope θ (see Figure 2). Here, Cf denotes the friction coefficient. Neglecting friction, (5.2) in generalized sense of association is given by
(5.3)ht+(hu)x~0,(5.4)(u)t+12(u2)x+g′hx~g′S.
Now, we assume that the depth has a jump in the bottom (see Figure 5). In this case, the bottom can be written as
(5.5)ho(x)=h1+(h2-h1)H(x),
where H is the Heaviside generalized function, and Δh=h2-h1 and h1, h2 are constants.


#### 5.1.1. A Case of Single Soliton

Givenτ1>0, we find a generalized solution of system (5.3) and (5.4) as
(5.6)η(x,t)=λSτ1(x-X(t)),u(x,t)=αSτ1(x-X(t)),
where X(t) is that trajectory of the singularities, and Sτ1 is the step generalized function. We assume that at time t=0, the generalized solution is known, that is,
(5.7)η(x,0)=λSτ1(x),u(x,0)=uoSτ1(x),
where λ and uo are known constants. The following theorem holds.Theorem 5.1.
It is assumed that solitons of the system (5.3) and (5.4) are given by
(5.8)η=λSτ1(x-X(t)),u=uoSτ1(x-X(t)),
for a given τ1, where λ and uo are constants representing the amplitude of surface elevation and particle velocity, respectively, and h=ho+η, where ho is given in (5.5). Here, X(t) is the trajectory where the singularity travels and let it be denoted by c1=X′(t) for x<0 and c2=X′(t) for x>0 the soliton velocity. Assuming that λ is known, then the soliton velocities c1, c2 are given by
(5.9)c1=uo(h1+λ)λ,c2=uo(h2+λ)λ.Proof.
Substituting (5.6) and (5.5) in (5.3) with ξ=x-X(t), we obtain
(5.10)-X′λSτ1′(ξ)+(uoSτ1(ξ))(Δhδ(x)+λSτ1′(ξ))+(h1+ΔhH(x)+λSτ1(ξ))uoSτ1′(ξ)~0.
Using that Sτ1′(ξ)Sτ1(ξ)~(1/2)(Sτ12(ξ))′, Lemma 3.2 and Lemma 3.3(i), that we have from (5.10)
(5.11)(-X′λ+12uoλ+uoh1+12uoλ+uoΔhH(x))Sτ1′(ξ)~0.
Since Sτ1′(ξ) is not associate to null generalized function, we obtain
(5.12)-X′λ+12uoλ+uoh1+12uoλ+uoΔhH(x)=0.
From (5.12), we obtain (5.9).Remark 5.2.
Theorem5.1 indicates that the trajectory of the singularity of one soliton that passes by the discontinuity point in the bottom consist in a cone. Moreover, the velocity of the soliton is constant and different in both sides of the jump. This suggests from the physical point of view that happened, a rectification of the soliton and velocity only depends on the depth.


#### 5.1.2. A Case of Two Solitons

Now, we obtain a solution of shallow water equation as two solitons which we assume are the propagate soliton, and reflected by the jump. Using the heuristic considerations despite in Remark5.2, we assume that the velocity of the solitons is constant.Givenτ1>0, we find a generalized solution of system (5.3) and (5.4) as
(5.13)η(x,t)=λ1Sτ1(x-c1t)+λ2Sτ1(x+c2t),u(x,t)=uo1Sτ1(x-c1t)+uo2Sτ1(x+c2t),
where c1, c2 are constants, and Sτ1 is the step generalized function. We assume that at time t=0, the generalized solution is known, that is,
(5.14)η(x,0)=(λ1+λ2)Sτ1(x)=λSτ1(x),u(x,0)=(uo1+uo2)Sτ1(x)=uoSτ1(x),
where λ=λ1+λ2 and uo=uo1+uo2 are considered as constants. In this case, we consider the discontinuous bottom as in (5.5). The following theorem holds.Theorem 5.3.
For givenτ1>0, let it be assumed that a generalized solution of (5.3) and (5.4) is given by (5.13) with bottom depth given in (5.5). Assuming that the amplitudes λ and uo are known, then the wave velocities c1 and c2, the amplitude of particle velocity uo2, and the amplitude λ2 of reflected wave satisfy on t>min{τ1/c1,τ1/c2} the following algebraic equations:
(5.15)-c1(λ-λ2)+(uo-uo2)[(λ-λ2)+h1+MΔh]=0,(5.16)λ2c2+uo2[λ2+h1]=0,(5.17)-c1(λ-λ2)+12(uo-uo2)2+g(λ-λ2)=0,(5.18)λ2c2+12uo22+gλ2=0,
where M is a constant.Proof.
Denote that byξ1=x-c1t and ξ2=x+c2t, we have
(5.19)η(x,t)=(λ-λ2)Sτ1(ξ1)+λ2Sτ1(ξ2),u(x,t)=(uo-uo2)Sτ1(ξ1)+uo2Sτ1(ξ2),h(x,t)=ho(x)+η(x,t).
Now, substituting (5.19) in (5.3) we obtain
(5.20)(ho(x))t+(-c1)(λ-λ2)Sτ1′(ξ1)+c2λ2Sτ1′(ξ2)+[(uo-uo2)Sτ1(ξ1)+uo2Sτ1(ξ2)][h1+ΔhH(x)]x+[(uo-uo2)Sτ1(ξ1)+uo2Sτ1(ξ2)][(λ-λ2)Sτ1′(ξ1)+λ2Sτ1′(ξ2)]+h(x,t)[(uo-uo2)Sτ1′(ξ1)+uo2Sτ1′(ξ2)]~0.
Now, using that Sτ1Sτ1′=(1/2)(Sτ12)′ and from Lemma 3.3 that Sτ1′(ξ1)Sτ1(ξ2)~0, Sτ1′(ξ2)Sτ1(ξ1)~0, we have
(5.21)-c1(λ-λ2)Sτ1′(ξ1)+c2λ2Sτ1′(ξ2)+Δh[(uo-uo2)Sτ1(ξ1)S(x)+uo2Sτ1(ξ2)S(x)]+[12(uo-uo2)(λ-λ2)(Sτ12(ξ1))′+12λ2uo2(Sτ12(ξ2))′]+h1[(uo-uo2)Sτ1′(ξ1)+uo2Sτ1′(ξ2)]+Δh[(uo-uo2)Sτ1′(ξ1)H(x)+uo2Sτ1′(ξ2)H(x)]+[12(λ-λ2)(uo-uo2)(Sτ12(ξ1))′+λ2uo2(Sτ12(ξ2))′]~0.
From Lemma 3.1, we have Sτ1′(ξ1)H(x)~MSτ1′(ξ1) and Sτ1′(ξ2)H(x)~0 for some constant M and for t,c>0. Also, from Lemma 3.2 we have Sτ1(ξ1)δ(x)~0 and Sτ1(ξ2)δ(x)~0 for c1,c2,t>0, and since Sτ12~Sτ1 (see Lemma 3.3(i)), we obtain
(5.22)[-c1(λ-λ2)+12(uo-uo2)(λ-λ2)+h1(uo-uo2)+MΔh(uo-uo2)+12(λ-λ2)(uo-uo2)]Sτ1′(ξ1)+[λ2c2+12uo2λ2+h1uo2+12λ2uo2]Sτ1′(ξ2)~0.
Analogously, substituting (5.19) in (5.4), we obtain
(5.23)-c1(λ-λ2)Sτ1′(ξ1)+c2uo2Sτ1′(ξ2)+((uo-uo2)Sτ1(ξ1)+uo2Sτ1(ξ2))((uo-uo2)Sτ1′(ξ1)+uo2S1′(ξ2))+g′[h1+ΔhH(x)]x+g′[(λ-λ2)Sτ1′(ξ1)+λ2Sτ1′(ξ2)]~g′tan(θ).
Now, from Lemma 3.3 (i), we have Sτ12~Sτ1. Also from Lemma 3.3(ii)(iii), we have Sτ1′(ξ1)Sτ1(ξ2)~0 and Sτ1(ξ1)Sτ1′(ξ2)~0 for t>min{τ1/c1,τ1/c2}. Since Sτ1Sτ1′=(1/2)(Sτ12)′, Sτ1(ξ1)δ1~0, Sτ1(ξ2)δ1~0 (Lemma 3.4(i)(ii)), we obtain
(5.24)g′ΔhH′+[-c1(λ-λ2)+12(uo-uo2)2+gcos⁡(θ)(λ-λ2)]Sτ1′(ξ1)+[uo2c1+12uo22+gcos⁡(θ)λ2]Sτ1′(ξ2)~g′tan⁡(θ).
Finally, using that cos(θ)~1-δ1(x) and tan(θ)~Δhδ, where θ is the angle in respect to axis OX (see (2.6) and (2.9)) and using Lemma 3.4, we have
(5.25)g′Δhδ+[-c1(λ-λ2)+12(uo-uo2)2+g(λ-λ2)]Sτ1′(ξ1)+[uo2c1+12uo22+gλ2]Sτ1′(ξ2)~g′Δhδ,
or equivalently,
(5.26)[-c1(λ-λ2)+12(uo-uo2)2+g(uo-uo2)]Sτ1′(ξ1)+[uo2c1+12uo22+gλ2]Sτ1′(ξ2)~0.
Because that the generalized function of the left hand of (5.22) and (5.26) is equivalent to zero, it is necessary that the coefficient of S1′(ξ1) and S1′(ξ2) must be zero. So, the system of (5.15)–(5.18) holds.Remark 5.4.
Although Theorem5.3 was obtained for a discontinuity in the bottom, it is not difficult to generalize this result for any type of bottom. To do so, any geometric of the bottom can be approximated by step functions, and then theorem can be used locally.Remark 5.5.
In Theorem5.3, we assume that t>min{τ1/c1,τ1/c2}. If we relax this hypothesis, that is, to obtain the generalized solution on 0<t<min{τ1/c1,τ1/c2}, we have that, following relations hold:
(5.27)Sτ1′(ξ1)Sτ1(ξ2)~δ(x-ct-τ1),Sτ1(ξ1)Sτ1′(ξ2)~-δ(x+ct+τ1),
where δ is the Dirac generalized function. The product of generalized functions (5.27) was taken as null in the proof of Theorem 5.3. In the contrary case, it is possible to check that in the proof (similar to Theorem 5.3), a new equation arises due to the coefficients of Sτ1′(ξ1)Sτ1(ξ2) and Sτ1(ξ1)Sτ1′(ξ2), which is
(5.28)(uo-uo2)uo2=0.
Equation (5.28) has two solutions which are uo=uo2 or uo2=0. More physical sense has the solution uo2=0, which means that for t<min{τ1/c1,τ1/c2}, the reflected effect of wave velocity particles is not starting yet. In this point, a rise of the wave amplitude near the leading edge of the discontinuous point occurs due to the shallow effect [51]. In that case it is possible to verify that system (5.15)–(5.18) reduces to the system of equations
(5.29)-c1λ+uo(λ+h1+MΔh)=0,-c1λ+gλ+12uo2=0.
Equation (5.29) for known λ has the explicit solutions:
(5.30)uo1,2=(h1+λ+MΔh)±(h1+λ+MΔh)2-2gλ,c11,2=-uo1,2h1+λ+MΔhλ,
with c2=λ2=uo2=0. However, taking off the amplitude wave λ of (5.29) and equaling it, we obtain
(5.31)uo/2(g-c1)=h1+MΔh(c1-uo).
Now, solving a close system (5.29), and (5.31), we obtain (c1,uo,λ), that is, wave celerity, particle velocity, and wave amplitude, respectively.


## 5.1. Generalized Solution

Following the same idea as in the previous section, we obtain a generalized solution of shallow water equation stated in [6] as in this case one takes into account friction and slope of the bottom
(5.1)ht+(hu)x=0,(5.2)(u)t+12(u2)x+g′hx=g′S-Cfu2,
where g′=gcos(θ), S=tan(θ) with bottom slope θ (see Figure 2). Here, Cf denotes the friction coefficient. Neglecting friction, (5.2) in generalized sense of association is given by
(5.3)ht+(hu)x~0,(5.4)(u)t+12(u2)x+g′hx~g′S.
Now, we assume that the depth has a jump in the bottom (see Figure 5). In this case, the bottom can be written as
(5.5)ho(x)=h1+(h2-h1)H(x),
where H is the Heaviside generalized function, and Δh=h2-h1 and h1, h2 are constants.


### 5.1.1. A Case of Single Soliton

Givenτ1>0, we find a generalized solution of system (5.3) and (5.4) as
(5.6)η(x,t)=λSτ1(x-X(t)),u(x,t)=αSτ1(x-X(t)),
where X(t) is that trajectory of the singularities, and Sτ1 is the step generalized function. We assume that at time t=0, the generalized solution is known, that is,
(5.7)η(x,0)=λSτ1(x),u(x,0)=uoSτ1(x),
where λ and uo are known constants. The following theorem holds.Theorem 5.1.
It is assumed that solitons of the system (5.3) and (5.4) are given by
(5.8)η=λSτ1(x-X(t)),u=uoSτ1(x-X(t)),
for a given τ1, where λ and uo are constants representing the amplitude of surface elevation and particle velocity, respectively, and h=ho+η, where ho is given in (5.5). Here, X(t) is the trajectory where the singularity travels and let it be denoted by c1=X′(t) for x<0 and c2=X′(t) for x>0 the soliton velocity. Assuming that λ is known, then the soliton velocities c1, c2 are given by
(5.9)c1=uo(h1+λ)λ,c2=uo(h2+λ)λ.Proof.
Substituting (5.6) and (5.5) in (5.3) with ξ=x-X(t), we obtain
(5.10)-X′λSτ1′(ξ)+(uoSτ1(ξ))(Δhδ(x)+λSτ1′(ξ))+(h1+ΔhH(x)+λSτ1(ξ))uoSτ1′(ξ)~0.
Using that Sτ1′(ξ)Sτ1(ξ)~(1/2)(Sτ12(ξ))′, Lemma 3.2 and Lemma 3.3(i), that we have from (5.10)
(5.11)(-X′λ+12uoλ+uoh1+12uoλ+uoΔhH(x))Sτ1′(ξ)~0.
Since Sτ1′(ξ) is not associate to null generalized function, we obtain
(5.12)-X′λ+12uoλ+uoh1+12uoλ+uoΔhH(x)=0.
From (5.12), we obtain (5.9).Remark 5.2.
Theorem5.1 indicates that the trajectory of the singularity of one soliton that passes by the discontinuity point in the bottom consist in a cone. Moreover, the velocity of the soliton is constant and different in both sides of the jump. This suggests from the physical point of view that happened, a rectification of the soliton and velocity only depends on the depth.


### 5.1.2. A Case of Two Solitons

Now, we obtain a solution of shallow water equation as two solitons which we assume are the propagate soliton, and reflected by the jump. Using the heuristic considerations despite in Remark5.2, we assume that the velocity of the solitons is constant.Givenτ1>0, we find a generalized solution of system (5.3) and (5.4) as
(5.13)η(x,t)=λ1Sτ1(x-c1t)+λ2Sτ1(x+c2t),u(x,t)=uo1Sτ1(x-c1t)+uo2Sτ1(x+c2t),
where c1, c2 are constants, and Sτ1 is the step generalized function. We assume that at time t=0, the generalized solution is known, that is,
(5.14)η(x,0)=(λ1+λ2)Sτ1(x)=λSτ1(x),u(x,0)=(uo1+uo2)Sτ1(x)=uoSτ1(x),
where λ=λ1+λ2 and uo=uo1+uo2 are considered as constants. In this case, we consider the discontinuous bottom as in (5.5). The following theorem holds.Theorem 5.3.
For givenτ1>0, let it be assumed that a generalized solution of (5.3) and (5.4) is given by (5.13) with bottom depth given in (5.5). Assuming that the amplitudes λ and uo are known, then the wave velocities c1 and c2, the amplitude of particle velocity uo2, and the amplitude λ2 of reflected wave satisfy on t>min{τ1/c1,τ1/c2} the following algebraic equations:
(5.15)-c1(λ-λ2)+(uo-uo2)[(λ-λ2)+h1+MΔh]=0,(5.16)λ2c2+uo2[λ2+h1]=0,(5.17)-c1(λ-λ2)+12(uo-uo2)2+g(λ-λ2)=0,(5.18)λ2c2+12uo22+gλ2=0,
where M is a constant.Proof.
Denote that byξ1=x-c1t and ξ2=x+c2t, we have
(5.19)η(x,t)=(λ-λ2)Sτ1(ξ1)+λ2Sτ1(ξ2),u(x,t)=(uo-uo2)Sτ1(ξ1)+uo2Sτ1(ξ2),h(x,t)=ho(x)+η(x,t).
Now, substituting (5.19) in (5.3) we obtain
(5.20)(ho(x))t+(-c1)(λ-λ2)Sτ1′(ξ1)+c2λ2Sτ1′(ξ2)+[(uo-uo2)Sτ1(ξ1)+uo2Sτ1(ξ2)][h1+ΔhH(x)]x+[(uo-uo2)Sτ1(ξ1)+uo2Sτ1(ξ2)][(λ-λ2)Sτ1′(ξ1)+λ2Sτ1′(ξ2)]+h(x,t)[(uo-uo2)Sτ1′(ξ1)+uo2Sτ1′(ξ2)]~0.
Now, using that Sτ1Sτ1′=(1/2)(Sτ12)′ and from Lemma 3.3 that Sτ1′(ξ1)Sτ1(ξ2)~0, Sτ1′(ξ2)Sτ1(ξ1)~0, we have
(5.21)-c1(λ-λ2)Sτ1′(ξ1)+c2λ2Sτ1′(ξ2)+Δh[(uo-uo2)Sτ1(ξ1)S(x)+uo2Sτ1(ξ2)S(x)]+[12(uo-uo2)(λ-λ2)(Sτ12(ξ1))′+12λ2uo2(Sτ12(ξ2))′]+h1[(uo-uo2)Sτ1′(ξ1)+uo2Sτ1′(ξ2)]+Δh[(uo-uo2)Sτ1′(ξ1)H(x)+uo2Sτ1′(ξ2)H(x)]+[12(λ-λ2)(uo-uo2)(Sτ12(ξ1))′+λ2uo2(Sτ12(ξ2))′]~0.
From Lemma 3.1, we have Sτ1′(ξ1)H(x)~MSτ1′(ξ1) and Sτ1′(ξ2)H(x)~0 for some constant M and for t,c>0. Also, from Lemma 3.2 we have Sτ1(ξ1)δ(x)~0 and Sτ1(ξ2)δ(x)~0 for c1,c2,t>0, and since Sτ12~Sτ1 (see Lemma 3.3(i)), we obtain
(5.22)[-c1(λ-λ2)+12(uo-uo2)(λ-λ2)+h1(uo-uo2)+MΔh(uo-uo2)+12(λ-λ2)(uo-uo2)]Sτ1′(ξ1)+[λ2c2+12uo2λ2+h1uo2+12λ2uo2]Sτ1′(ξ2)~0.
Analogously, substituting (5.19) in (5.4), we obtain
(5.23)-c1(λ-λ2)Sτ1′(ξ1)+c2uo2Sτ1′(ξ2)+((uo-uo2)Sτ1(ξ1)+uo2Sτ1(ξ2))((uo-uo2)Sτ1′(ξ1)+uo2S1′(ξ2))+g′[h1+ΔhH(x)]x+g′[(λ-λ2)Sτ1′(ξ1)+λ2Sτ1′(ξ2)]~g′tan(θ).
Now, from Lemma 3.3 (i), we have Sτ12~Sτ1. Also from Lemma 3.3(ii)(iii), we have Sτ1′(ξ1)Sτ1(ξ2)~0 and Sτ1(ξ1)Sτ1′(ξ2)~0 for t>min{τ1/c1,τ1/c2}. Since Sτ1Sτ1′=(1/2)(Sτ12)′, Sτ1(ξ1)δ1~0, Sτ1(ξ2)δ1~0 (Lemma 3.4(i)(ii)), we obtain
(5.24)g′ΔhH′+[-c1(λ-λ2)+12(uo-uo2)2+gcos⁡(θ)(λ-λ2)]Sτ1′(ξ1)+[uo2c1+12uo22+gcos⁡(θ)λ2]Sτ1′(ξ2)~g′tan⁡(θ).
Finally, using that cos(θ)~1-δ1(x) and tan(θ)~Δhδ, where θ is the angle in respect to axis OX (see (2.6) and (2.9)) and using Lemma 3.4, we have
(5.25)g′Δhδ+[-c1(λ-λ2)+12(uo-uo2)2+g(λ-λ2)]Sτ1′(ξ1)+[uo2c1+12uo22+gλ2]Sτ1′(ξ2)~g′Δhδ,
or equivalently,
(5.26)[-c1(λ-λ2)+12(uo-uo2)2+g(uo-uo2)]Sτ1′(ξ1)+[uo2c1+12uo22+gλ2]Sτ1′(ξ2)~0.
Because that the generalized function of the left hand of (5.22) and (5.26) is equivalent to zero, it is necessary that the coefficient of S1′(ξ1) and S1′(ξ2) must be zero. So, the system of (5.15)–(5.18) holds.Remark 5.4.
Although Theorem5.3 was obtained for a discontinuity in the bottom, it is not difficult to generalize this result for any type of bottom. To do so, any geometric of the bottom can be approximated by step functions, and then theorem can be used locally.Remark 5.5.
In Theorem5.3, we assume that t>min{τ1/c1,τ1/c2}. If we relax this hypothesis, that is, to obtain the generalized solution on 0<t<min{τ1/c1,τ1/c2}, we have that, following relations hold:
(5.27)Sτ1′(ξ1)Sτ1(ξ2)~δ(x-ct-τ1),Sτ1(ξ1)Sτ1′(ξ2)~-δ(x+ct+τ1),
where δ is the Dirac generalized function. The product of generalized functions (5.27) was taken as null in the proof of Theorem 5.3. In the contrary case, it is possible to check that in the proof (similar to Theorem 5.3), a new equation arises due to the coefficients of Sτ1′(ξ1)Sτ1(ξ2) and Sτ1(ξ1)Sτ1′(ξ2), which is
(5.28)(uo-uo2)uo2=0.
Equation (5.28) has two solutions which are uo=uo2 or uo2=0. More physical sense has the solution uo2=0, which means that for t<min{τ1/c1,τ1/c2}, the reflected effect of wave velocity particles is not starting yet. In this point, a rise of the wave amplitude near the leading edge of the discontinuous point occurs due to the shallow effect [51]. In that case it is possible to verify that system (5.15)–(5.18) reduces to the system of equations
(5.29)-c1λ+uo(λ+h1+MΔh)=0,-c1λ+gλ+12uo2=0.
Equation (5.29) for known λ has the explicit solutions:
(5.30)uo1,2=(h1+λ+MΔh)±(h1+λ+MΔh)2-2gλ,c11,2=-uo1,2h1+λ+MΔhλ,
with c2=λ2=uo2=0. However, taking off the amplitude wave λ of (5.29) and equaling it, we obtain
(5.31)uo/2(g-c1)=h1+MΔh(c1-uo).
Now, solving a close system (5.29), and (5.31), we obtain (c1,uo,λ), that is, wave celerity, particle velocity, and wave amplitude, respectively.


## 5.1.1. A Case of Single Soliton

Givenτ1>0, we find a generalized solution of system (5.3) and (5.4) as
(5.6)η(x,t)=λSτ1(x-X(t)),u(x,t)=αSτ1(x-X(t)),
where X(t) is that trajectory of the singularities, and Sτ1 is the step generalized function. We assume that at time t=0, the generalized solution is known, that is,
(5.7)η(x,0)=λSτ1(x),u(x,0)=uoSτ1(x),
where λ and uo are known constants. The following theorem holds.Theorem 5.1.
It is assumed that solitons of the system (5.3) and (5.4) are given by
(5.8)η=λSτ1(x-X(t)),u=uoSτ1(x-X(t)),
for a given τ1, where λ and uo are constants representing the amplitude of surface elevation and particle velocity, respectively, and h=ho+η, where ho is given in (5.5). Here, X(t) is the trajectory where the singularity travels and let it be denoted by c1=X′(t) for x<0 and c2=X′(t) for x>0 the soliton velocity. Assuming that λ is known, then the soliton velocities c1, c2 are given by
(5.9)c1=uo(h1+λ)λ,c2=uo(h2+λ)λ.Proof.
Substituting (5.6) and (5.5) in (5.3) with ξ=x-X(t), we obtain
(5.10)-X′λSτ1′(ξ)+(uoSτ1(ξ))(Δhδ(x)+λSτ1′(ξ))+(h1+ΔhH(x)+λSτ1(ξ))uoSτ1′(ξ)~0.
Using that Sτ1′(ξ)Sτ1(ξ)~(1/2)(Sτ12(ξ))′, Lemma 3.2 and Lemma 3.3(i), that we have from (5.10)
(5.11)(-X′λ+12uoλ+uoh1+12uoλ+uoΔhH(x))Sτ1′(ξ)~0.
Since Sτ1′(ξ) is not associate to null generalized function, we obtain
(5.12)-X′λ+12uoλ+uoh1+12uoλ+uoΔhH(x)=0.
From (5.12), we obtain (5.9).Remark 5.2.
Theorem5.1 indicates that the trajectory of the singularity of one soliton that passes by the discontinuity point in the bottom consist in a cone. Moreover, the velocity of the soliton is constant and different in both sides of the jump. This suggests from the physical point of view that happened, a rectification of the soliton and velocity only depends on the depth.


## 5.1.2. A Case of Two Solitons

Now, we obtain a solution of shallow water equation as two solitons which we assume are the propagate soliton, and reflected by the jump. Using the heuristic considerations despite in Remark5.2, we assume that the velocity of the solitons is constant.Givenτ1>0, we find a generalized solution of system (5.3) and (5.4) as
(5.13)η(x,t)=λ1Sτ1(x-c1t)+λ2Sτ1(x+c2t),u(x,t)=uo1Sτ1(x-c1t)+uo2Sτ1(x+c2t),
where c1, c2 are constants, and Sτ1 is the step generalized function. We assume that at time t=0, the generalized solution is known, that is,
(5.14)η(x,0)=(λ1+λ2)Sτ1(x)=λSτ1(x),u(x,0)=(uo1+uo2)Sτ1(x)=uoSτ1(x),
where λ=λ1+λ2 and uo=uo1+uo2 are considered as constants. In this case, we consider the discontinuous bottom as in (5.5). The following theorem holds.Theorem 5.3.
For givenτ1>0, let it be assumed that a generalized solution of (5.3) and (5.4) is given by (5.13) with bottom depth given in (5.5). Assuming that the amplitudes λ and uo are known, then the wave velocities c1 and c2, the amplitude of particle velocity uo2, and the amplitude λ2 of reflected wave satisfy on t>min{τ1/c1,τ1/c2} the following algebraic equations:
(5.15)-c1(λ-λ2)+(uo-uo2)[(λ-λ2)+h1+MΔh]=0,(5.16)λ2c2+uo2[λ2+h1]=0,(5.17)-c1(λ-λ2)+12(uo-uo2)2+g(λ-λ2)=0,(5.18)λ2c2+12uo22+gλ2=0,
where M is a constant.Proof.
Denote that byξ1=x-c1t and ξ2=x+c2t, we have
(5.19)η(x,t)=(λ-λ2)Sτ1(ξ1)+λ2Sτ1(ξ2),u(x,t)=(uo-uo2)Sτ1(ξ1)+uo2Sτ1(ξ2),h(x,t)=ho(x)+η(x,t).
Now, substituting (5.19) in (5.3) we obtain
(5.20)(ho(x))t+(-c1)(λ-λ2)Sτ1′(ξ1)+c2λ2Sτ1′(ξ2)+[(uo-uo2)Sτ1(ξ1)+uo2Sτ1(ξ2)][h1+ΔhH(x)]x+[(uo-uo2)Sτ1(ξ1)+uo2Sτ1(ξ2)][(λ-λ2)Sτ1′(ξ1)+λ2Sτ1′(ξ2)]+h(x,t)[(uo-uo2)Sτ1′(ξ1)+uo2Sτ1′(ξ2)]~0.
Now, using that Sτ1Sτ1′=(1/2)(Sτ12)′ and from Lemma 3.3 that Sτ1′(ξ1)Sτ1(ξ2)~0, Sτ1′(ξ2)Sτ1(ξ1)~0, we have
(5.21)-c1(λ-λ2)Sτ1′(ξ1)+c2λ2Sτ1′(ξ2)+Δh[(uo-uo2)Sτ1(ξ1)S(x)+uo2Sτ1(ξ2)S(x)]+[12(uo-uo2)(λ-λ2)(Sτ12(ξ1))′+12λ2uo2(Sτ12(ξ2))′]+h1[(uo-uo2)Sτ1′(ξ1)+uo2Sτ1′(ξ2)]+Δh[(uo-uo2)Sτ1′(ξ1)H(x)+uo2Sτ1′(ξ2)H(x)]+[12(λ-λ2)(uo-uo2)(Sτ12(ξ1))′+λ2uo2(Sτ12(ξ2))′]~0.
From Lemma 3.1, we have Sτ1′(ξ1)H(x)~MSτ1′(ξ1) and Sτ1′(ξ2)H(x)~0 for some constant M and for t,c>0. Also, from Lemma 3.2 we have Sτ1(ξ1)δ(x)~0 and Sτ1(ξ2)δ(x)~0 for c1,c2,t>0, and since Sτ12~Sτ1 (see Lemma 3.3(i)), we obtain
(5.22)[-c1(λ-λ2)+12(uo-uo2)(λ-λ2)+h1(uo-uo2)+MΔh(uo-uo2)+12(λ-λ2)(uo-uo2)]Sτ1′(ξ1)+[λ2c2+12uo2λ2+h1uo2+12λ2uo2]Sτ1′(ξ2)~0.
Analogously, substituting (5.19) in (5.4), we obtain
(5.23)-c1(λ-λ2)Sτ1′(ξ1)+c2uo2Sτ1′(ξ2)+((uo-uo2)Sτ1(ξ1)+uo2Sτ1(ξ2))((uo-uo2)Sτ1′(ξ1)+uo2S1′(ξ2))+g′[h1+ΔhH(x)]x+g′[(λ-λ2)Sτ1′(ξ1)+λ2Sτ1′(ξ2)]~g′tan(θ).
Now, from Lemma 3.3 (i), we have Sτ12~Sτ1. Also from Lemma 3.3(ii)(iii), we have Sτ1′(ξ1)Sτ1(ξ2)~0 and Sτ1(ξ1)Sτ1′(ξ2)~0 for t>min{τ1/c1,τ1/c2}. Since Sτ1Sτ1′=(1/2)(Sτ12)′, Sτ1(ξ1)δ1~0, Sτ1(ξ2)δ1~0 (Lemma 3.4(i)(ii)), we obtain
(5.24)g′ΔhH′+[-c1(λ-λ2)+12(uo-uo2)2+gcos⁡(θ)(λ-λ2)]Sτ1′(ξ1)+[uo2c1+12uo22+gcos⁡(θ)λ2]Sτ1′(ξ2)~g′tan⁡(θ).
Finally, using that cos(θ)~1-δ1(x) and tan(θ)~Δhδ, where θ is the angle in respect to axis OX (see (2.6) and (2.9)) and using Lemma 3.4, we have
(5.25)g′Δhδ+[-c1(λ-λ2)+12(uo-uo2)2+g(λ-λ2)]Sτ1′(ξ1)+[uo2c1+12uo22+gλ2]Sτ1′(ξ2)~g′Δhδ,
or equivalently,
(5.26)[-c1(λ-λ2)+12(uo-uo2)2+g(uo-uo2)]Sτ1′(ξ1)+[uo2c1+12uo22+gλ2]Sτ1′(ξ2)~0.
Because that the generalized function of the left hand of (5.22) and (5.26) is equivalent to zero, it is necessary that the coefficient of S1′(ξ1) and S1′(ξ2) must be zero. So, the system of (5.15)–(5.18) holds.Remark 5.4.
Although Theorem5.3 was obtained for a discontinuity in the bottom, it is not difficult to generalize this result for any type of bottom. To do so, any geometric of the bottom can be approximated by step functions, and then theorem can be used locally.Remark 5.5.
In Theorem5.3, we assume that t>min{τ1/c1,τ1/c2}. If we relax this hypothesis, that is, to obtain the generalized solution on 0<t<min{τ1/c1,τ1/c2}, we have that, following relations hold:
(5.27)Sτ1′(ξ1)Sτ1(ξ2)~δ(x-ct-τ1),Sτ1(ξ1)Sτ1′(ξ2)~-δ(x+ct+τ1),
where δ is the Dirac generalized function. The product of generalized functions (5.27) was taken as null in the proof of Theorem 5.3. In the contrary case, it is possible to check that in the proof (similar to Theorem 5.3), a new equation arises due to the coefficients of Sτ1′(ξ1)Sτ1(ξ2) and Sτ1(ξ1)Sτ1′(ξ2), which is
(5.28)(uo-uo2)uo2=0.
Equation (5.28) has two solutions which are uo=uo2 or uo2=0. More physical sense has the solution uo2=0, which means that for t<min{τ1/c1,τ1/c2}, the reflected effect of wave velocity particles is not starting yet. In this point, a rise of the wave amplitude near the leading edge of the discontinuous point occurs due to the shallow effect [51]. In that case it is possible to verify that system (5.15)–(5.18) reduces to the system of equations
(5.29)-c1λ+uo(λ+h1+MΔh)=0,-c1λ+gλ+12uo2=0.
Equation (5.29) for known λ has the explicit solutions:
(5.30)uo1,2=(h1+λ+MΔh)±(h1+λ+MΔh)2-2gλ,c11,2=-uo1,2h1+λ+MΔhλ,
with c2=λ2=uo2=0. However, taking off the amplitude wave λ of (5.29) and equaling it, we obtain
(5.31)uo/2(g-c1)=h1+MΔh(c1-uo).
Now, solving a close system (5.29), and (5.31), we obtain (c1,uo,λ), that is, wave celerity, particle velocity, and wave amplitude, respectively.


## 6. Numerical Calculation of the Generalized Solution

In this section, we show a numerical procedure to find the unknown parametersλ2 and uo2 which are solution of the system of (5.15)–(5.18). In practical terms to determine those parameters means to calculate the amplitude of the step Soliton when it passes through a point of discontinuity in the bottom. The method consists in reducing the set of four equations to two by eliminating the unknowns c1 and c2. The following lemma holds.Lemma 6.1.
Let it be assumed that a generalized solutions of (5.3) and (5.4) is given by (5.13) with bottom depth given in (5.5). Assuming that λ and uo are known, then the amplitude of particle velocity uo2 and the amplitude λ2 of the reflected wave satisfy
(6.1)12uo22-λ2uo2+gλ2-uo2h1=0,(6.2)12(uo-uo2)2-(λ-λ2)(uo-uo2)+g(λ-λ2)-(uo-uo2)(h1+MΔh)=0,
where M is a constant.Proof.
Equation (6.1) follows from (5.18) minus (5.16). Equation (6.2) follows from (5.17) minus (5.15).Let us denote(6.3)G1(uo2,λ2)=12uo22-λ2uo2+gλ2-uo2h1,G2(uo2,λ2)=12(uo-uo2)2-(λ-λ2)(uo-uo2)+g(λ-λ2)-(uo-uo2)(h1+MΔh).
Now, to find the zeros of (6.1) and (6.2) is equivalent to find the zeros of the application
(6.4)G:(uo2,λ2)⟶(G1(uo2,λ2),G2(uo2,λ2)),
in the region B={(uo2,λ2):0<uo2<uo and 0<λ2<λ}. To do so, it is possible to use the quasi-Newton method.Remark 6.2.
Takinguo2=0, λ2=0, and Δh=0, that is, the flat bottom case, then it is possible to verify that (6.1) and (6.2) is the same as the flat bottom case (4.4a) and (4.4b), which indicates that the calculation in the discontinuous bottom case is consistent.


## 7. Numerical Examples

In this section, we show that the generalized solutions with physical sense can be obtained. To do so, the constantM in the system of (5.15)–(5.18) can be adjusted such that generalized solutions represent appropriately the theoretical and experimental data.The initial values of quasi-Newton method for solving (6.1)-(6.2) are taken by using the formula for planar bottom case; that is, assuming the wave celerity is known from (4.4a) and (4.4b), we obtain gλ2+(2gho-(c2/2))λ+(gho2-hoc2)=0. It is possible to check that the positive root of the above equation produces a wave amplitude with reasonable value.In [45, 58] was used the theoretical amplitude of soliton λ1 in the impermeable case with a discontinuity bottom which was deduced in [45], which is
(7.1)λ1-1/4=λ-1/4+0.08356υg1/2h22(xh2),
where λ is the initial amplitude, x is the distance traveled by the soliton wave, and υ is the kinematic viscosity of the fluid. In [40], numerical results solving the Navier-Stokes equation match with the above theoretical result. The formula (7.1) to prove that the soliton generalized solution approximates the theoretical result is used in this paper.We take the example described in [40] which considered the discontinuity bottom as h1=80 cm, h2=40 cm, and the initial amplitude λ=4 cm. The theoretical result for this case using the formula (7.1) is compared with numerical solution of the system of (5.15)–(5.18). To approximate the theoretical solution, we present the generalized solution assuming that the constant M in system of (6.1)-(6.2) depends on x/h2, that is, M=M(x/h2). This assumption enables us to show that the solution of (5.15)–(5.18) can reproduce well several amplitude step soliton values above the break point. We seek the values of the M(x/h2) that better adjusted the theoretical amplitude in (7.1) (see Figure 6). To do so, we use the solver fmincon.m in MATLAB 7.0. In Figure 6 is shows the theoretical and predicted step soliton amplitude when pass on a discontinuous depth point (x=0).Figure 6
Theoretical and predicted amplitude wave of the soliton propagating over a discontinued bed. The pointx=0 coincides with the discontinuous bottom point.In [46] was performed experiments to investigate the harmonic generation as periodic waves propagate over a submerged porous breakwater. Their experimental data will be used to test the validation of the present model equations for the wave and discontinuous bottom point interaction. We check that the generalized solution can reproduce well this experimental values.Although we have been adjusted the method well to both theoretic and experimental data, this result constitutes a first approximation of application of Colombeau’s algebra, because we consider as a constant in time and space the amplitude of step soliton generalized function. Also, we do not consider here the friction effect and the time dependency amplitude wave. An other facility is that the parameterM that appears in (5.15) can be estimated from several experimental runs looking for any regularity.


## 8. Conclusion

In this paper generalized solutions in the sense of Colombeau of Shallow water equations are obtained. This solution is consistent with numerical and theoretical results of a soliton passing over a flat or discontinuity bottom geometries. The method developed in this paper reduces the partial differential equation to determine the zeros of a functional equation. This procedure also will allow us to study a propagation of several types of singularities on several bottom geometries.



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*Source: 910659-2012-07-26.xml*