# Analytical Solutions for Two Mixed Initial-Boundary Value Problems Corresponding to Unsteady Motions of Maxwell Fluids through a Porous Plate Channel

Authors: Constantin Fetecau; Dumitru Vieru; Ahmed Zeeshan
Journal: Mathematical Problems in Engineering
 (2021)

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## Abstract

Two unsteady motions of incompressible Maxwell fluids between infinite horizontal parallel plates embedded in a porous medium are analytically studied to get exact solutions using the finite Fourier cosine transform. The motion is induced by the lower plate that applies time-dependent shear stresses to the fluid. The solutions that have been obtained satisfy all imposed initial and boundary conditions. They can be easily reduced as limiting cases to known solutions for the incompressible Newtonian fluids. For a check of their correctness, the steady-state solutions are presented in different forms whose equivalence is graphically proved. The effects of physical parameters on the fluid motion are graphically emphasized and discussed. Required time to reach the steady-state is also determined. It is found that the steady-state is rather obtained for Newtonian fluids as compared with Maxwell fluids. Furthermore, the effect of the side walls on the fluid motion is more effective in the case of Newtonian fluids.


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## Body

## 1. Introduction

Exact solutions for initial and boundary value problems are important for many reasons. First of all, they can characterize the behavior of some fluids or solids in various circumstances. Secondly, they can be used as tests to verify numerical schemes which are implemented to study more complex deformation or motion problems. Although the numerical integration of the differential or integral equations can be realized by computers, the accuracy of results is easier established comparing with exact solutions. During the time, many exact solutions have been established for motions of the Newtonian and non-Newtonian fluids in different circumstances (see, for instance, [1, 2] for flows between two parallel plates). Generally, they correspond to initial and boundary value problems in which the velocity is given on the boundary although in some practical situations the shear stress is specified on the solid wall.Relatively in recent studies, Renardy [3] mentioned that boundary conditions on stresses have to be imposed to formulate a well-posed boundary value problem for the flow of a Maxwell fluid between parallel plates. He also considered steady flows of viscoelastic fluids [4] and showed that the Jeffrey model is well-posed in a bounded channel if the extra-stress components are given on the boundary. Actually, in the Newtonian mechanics, the force is the cause and kinematics is the effect and prescribing the shear stress on the boundary is the same to prescribe the force applied to the boundary in order to move it [5]. The first exact solutions for motions of non-Newtonian fluids in which the shear stress is given on the boundary have been obtained by Ting [6] and Waters and King [7], respectively, for flows of second grade or Oldroyd-B fluids over an infinite plate. First exact solutions for unsteady motions of non-Newtonian fluids in which the shear stress is given on a portion of the boundary and the velocity on the other part of the boundary seem to be those of Bandelli and Rajagopal [8] for flows of the second grade fluids in cylindrical domains.In the meantime, different exact solutions for such motions of the non-Newtonian fluids were determined both in rectangular and cylindrical domains (see, for instance, [9–15] and the references therein). General solutions for the motion of Newtonian fluids between parallel plates in which the shear stress is given on a part of the boundary were recently determined by Javaid et al. [16]. Other exact solutions for such motions of the incompressible Newtonian fluids with pressure-dependent viscosity were recently provided by Danish et al. [17]. Exact expressions for the steady-state solutions corresponding to oscillatory motions of the Maxwell fluids in long tubes of rectangular or triangular cross section were recently obtained by Wang et al. [18] and Sun et al. [19], respectively. Starting solutions for nonsteady flows of the Maxwell fluids induced by a moving wall through a porous plate channel were recently provided by Fetecau et al. [20]. An interesting study concerning the Maxwell fluid flow through porous plate was developed by Shahid [21]. To the best of our knowledge, closed-form expressions for starting solutions corresponding to mixed initial-boundary value problems of the Maxwell fluids moving in a porous medium lack in the literature.The purpose of this note is to provide analytical expressions for two unsteady motions of incompressible Maxwell fluids through a horizontal porous plate channel. The fluid motion is generated by the lower plate that applies time-dependent shear stresses to the fluid. Obtained solutions fulfill all imposed initial and boundary conditions and are easily reduced to known solutions for the Newtonian fluids. For validation, the steady-state solutions are presented in different forms and their equivalence is graphically proved. Effects of pertinent parameters on the fluid movement are graphically underlined and interpreted. The required time to reach the steady-state is graphically determined. It is found that the steady-state is later obtained for Maxwell fluids as compared with Newtonian fluids. Furthermore, the effect of the side walls on the fluid motion is more effective on Newtonian fluids than the Maxwell fluids.


## 2. Statement of the Problem

Let us consider an incompressible upper-convected Maxwell (UCM) fluid between two infinite horizontal parallel plates embedded in a porous medium as illustrated in Figure1.Figure 1
Geometry of the flow.The constitutive equations of such a fluid are as follows [22]:(1)T=−pI+S,S+λdSdt−LS−SLT=μL+LT,where T is the Cauchy stress tensor, S is the extra-stress tensor, −pI is the constitutively indeterminate part of the stress due to the constraint of incompressibility, λ is the relaxation time, μ is the fluid viscosity, and L is the gradient of the velocity field v. In the following, we establish exact solutions for two mixed initial-boundary value problems corresponding to unsteady motions of incompressible UCM fluids into abovementioned domain. All results will be reported to a convenient Cartesian coordinate system having the y-axis perpendicular to plates.Since the plates are infinite in extent, all physical entities which characterize the fluid motion in such a domain are functions ofy and t only [23]. Consequently, for such motions of the incompressible UCM fluids, we can look for a velocity field of the form as follows:(2)v=vy,t=uy,tex,where ex is the unit vector along the x-direction. We also suppose that the extra-stress tensor S, as well as the fluid velocity v, depends on y and t only.Replacing the above velocity field in the constitutive equation (1) and bearing in mind the fact that the fluid was at rest up to the moment t=0, i.e.,(3)vy,0=0,Sy,0=0,it can be proved that the components Sxz,Syz,Syy, and Szz of S are zero and [20](4)τy,t+λ∂τy,t∂t=μ∂uy,t∂y,σy,t+λ∂σy,t∂t=2λτy,t∂uy,t∂y,where τy,t=Sxyy,t and σy,t=Sxxy,t are the non-null components of S.Let us now assume that at the momentt=0+, the lower plate begins to apply to the fluid a shear stress τ0,t having one of the forms as follows:(5)τ0,t=S1t−λ1−exp−tλ,τ0,t=S2sinωt−λωcosωtλω2+1+λωS2λω2+1exp−tλ,where S1 and S2 are dimensional constants. In the case λ⟶0, corresponding to Newtonian fluids, the above relations take the simple forms as follows:(6)τ0,t=S1t,respectivelyτ0,t=S2sinωt.Boundary conditions of same forms (6), but for the velocity components, have been recently used by Wang and Liu (see Section 3 in [24]) for the helical flow of generalized Maxwell fluids.Due to the shear, the fluid begins to move and, in the absence of a pressure gradient in thex-direction, the balance of linear momentum reduces to the partial differential equation as follows [25]:(7)ρ∂uy,t∂t=∂τy,t∂y+Ry,t,where Ry,t is Darcy’s resistance which for such fluids has to satisfy the following relation:(8)Ry,t+λ∂Ry,t∂t=−μϕkuy,t.In the above relations,ρ is the fluid density while ϕ and k are the porosity and the permeability, respectively, of the porous medium. The continuity equation is identically satisfied.Eliminatingτy,t between equations (4) and (7) and using equation (8), one attains the following dimensional governing equation for the velocity field:(9)λ∂2uy,t∂t2+∂uy,t∂t=ν∂2uy,t∂y2−νϕkuy,t;0<y<d,t>0,in which ν=μ/ρ is the kinematic viscosity and d is the distance between plates.The appropriate initial and boundary conditions are(10)uy,0=0,∂uy,t∂t|t=0=0;0≤y≤d,(11)τ0,t+λ∂τ0,t∂t=μ∂uy,t∂y|y=0=S1t,ud,t=0ift>0,for the first motion, and the initial conditions (10) together with the boundary conditions are as follows:(12)τ0,t+λ∂τ0,t∂t=μ∂uy,t∂y|y=0=S2sinωt,ud,t=0ift>0,in the case of the second motion. It is worth to point out the fact that solving the ordinary differential equations (11) and (12) with respect to τ0,t when the initial condition τ0,0=0 resulting from equation (3) is satisfied, and equality (5) is recovered.As soon as the velocity fielduy,t is known, the shear and normal stresses τy,t and σy,t can be determined solving the governing equation (4) with the initial conditions as follows:(13)τy,0=0,σy,0=0;0≤y≤d.However, in order to avoid repetition, we shall here determine the shear stressτy,t only. It is necessary, for instance, to provide the frictional force per unit area exerted by the fluid on the stationary plate.


## 3. Solution

In the following, the finite Fourier cosine transform, defined by equation (A.1) from Appendix, is used to determine analytical expressions for the dimensionless velocity and shear stress fields corresponding to the two unsteady motions of the incompressible UCM fluids through a porous plate channel.


### 3.1. Caseτ0,t=S1t−λ1−exp−t/λ

In order to determine solutions which are independent of the flow geometry, let us introduce the following nondimensional variables and functions:(14)y∗=yd,t∗=νd2t,u∗=μνd3S1u,τ∗=νd2S1τ,σ∗=νd2S1σ.Introducing the above nondimensional entities in equations (9)–(11) and giving up the star notation, the next mixed initial-boundary value problem(15)We∂2uy,t∂t2+∂uy,t∂t=∂2uy,t∂y2−Kuy,t;0<y<1,t>0,(16)uy,0=0,∂uy,t∂t|t=0=0for0≤y≤1,(17)∂uy,t∂y|y=0=t,u1,0=0ift>0,is obtained. In equation (15), the Weissenberg number We and the dimensionless porosity parameter K are defined by the equalities as follows:(18)We=λVd,K=ϕkd2,where V=ν/d is a characteristic velocity. The Weissenberg number We represents the ratio of the relaxation time λ and the characteristic time t0=d/V.The dimensionless forms of the ordinary differential equation (4) are(19)We∂τy,t∂t+τy,t=∂uy,t∂y,We∂σy,t∂t+σy,t=2ατy,t∂uy,t∂y;0<y<1,t>0,where α=λd2S1/μν. The corresponding initial conditions are(20)τy,0=0andσy,0=0;0≤y≤1.Multiplying equation (15) with cosμny, where μn=2n+1π/2, integrating the result from zero to one, and bearing in mind the initial and boundary conditions (16) and (17) and equalities (A.1) and (A.2) from Appendix, it results that the finite Fourier cosine transform uFnt of uy,t has to satisfy the ordinary differential equation as follows:(21)Wed2uFntdt2+duFntdt+μn2+KuFnt=−t;t>0,n=1,2,3...,with the initial conditions(22)uFn0=0,duFntdt|t=0=0;n=1,2,3...The solution of equation (21) with the initial conditions (22) is given by the relation as follows:(23)uFnt=1an−t+1an+an+r1ner2nt−an+r2ner1ntr2n−r1nan;n=1,2,3...,where an=μn2+K and r1n,2n=−1±1−4Wean/2We. On the basis of equality (A.1),it results that the dimensionless velocity field uy,t corresponding to this motion is given by(24)uy,t=2∑n=0∞−t+1an+an+r1ner2nt−an+r2ner1ntr2n−r1nancosμnyan;0<y<1,t>0,or equivalently (see the equality (A.3) from Appendix)(25)uy,t=y−1t+2tK∑n=0∞cosμnyanμn2+2∑n=0∞1+an+r1ner2nt−an+r2ner1ntr2n−r1ncosμnyan2.Direct computations clearly show thatuy,t given by equality (25) satisfies both the governing equation (15) and all imposed initial and boundary conditions. The dimensionless volume flux across a plane normal to the x-axis and per unit width of this plane is given by the relation as follows:(26)Q=Qt=−t2+2tK∑n=0∞−1nμn3μn2+K+2∑n=0∞1+an+r1ner2nt−an+r2ner1ntr2n−r1n−1nμn2+K2.Fort=0, as expected, Q becomes zero.In order to determine the dimensionless frictional force per unit area exerted by the fluid on the stationary plate, the corresponding shear stressτy,t has to be known. Replacing the expression of uy,t from equality (25) in (19) and solving the obtained equation with the initial condition (20), it results that τy,t is given by the following expression:(27)τy,t=t−We1−exp−tWe1−2K∑n=0∞sinμnyμnμn2+K−2∑n=0∞1+an+r1nWer1n+1er2nt−an+r2nWer2n+1er1ntr2n−r1nWer1n+1Wer2n+1μnsinμnyμn2+K2+2exp−tWe∑n=0∞1+an+r1nWer1n+1−an+r2nWer2n+1r2n−r1nWer1n+1Wer2n+1μnsinμnyμn2+K2.The motion whose solutions have been determined in this subsection is unsteady and remains unsteady. It is clear that at large enough values of the timet, the fluid motion can be described by the long time solutions:(28)uLty,t=y−1t+2tK∑n=0∞cosμnyμn2μn2+K+2∑n=0∞cosμnyμn2+K2,(29)τLty,t=t−We1−2K∑n=0∞sinμnyμnμn2+K−2∑n=0∞μnsinμnyμn2+K2.As expected, the dimensionless velocity and shear stress fieldsuNy,t and τNy,t corresponding to incompressible Newtonian fluids performing the same motion, namely, (30)uNy,t=y−1t+2tK∑n=0∞cosμnyμn2μn2+K+2∑n=0∞1−e−μn2+Ktcosμnyμn2+K2,(31)τNy,t=t−2tK∑n=0∞sinμnyμnμn2+K−2∑n=0∞1−e−μn2+Ktμnsinμnyμn2+K2,are immediately obtained making We⟶0 in equations (25) and (27). Of course, the last solutions are in agreement with the solutions obtained in equalities (29) and (31) in [16] where the boundary condition (8) has been taken with a changed sign. The corresponding volume flux QN can be immediately obtained making We=0 in the general expression of Q. In the absence of the porous effects, the corresponding solutions can be determined making K⟶0 into the above relations.From equalities (28) and (30), it clearly results that the long time velocity fields uLty,t and uNLty,t corresponding to the incompressible UCM and Newtonian fluids, respectively, are identical. Consequently, for large enough values of the time t, the dimensionless velocity field uLty,t corresponding to incompressible UCM fluids can be approximated with that of Newtonian fluids. Of course, bearing in mind known results from the existing literature, this is not a surprise. However, this property is not valid for the corresponding shear stress fields. The corresponding frictional forces per unit area exerted by the fluid on the upper plate can be immediately determined making y=1 in any one of the relations (27), (29), or (31).


### 3.2. Caseτ0,t=S2sinωt−λωcosωt−exp−t/λ/λω2+1

Introducing the next nondimensional variables, functions, and parameters such as(32)y∗=yd,t∗=νd2t,u∗=μdS2u,τ∗=τS2,σ∗=σS2,ω∗=d2νωin equality (9) and again dropping out the star notation, one obtains for the velocity field usy,t corresponding to this motion a dimensionless governing equation of the same form as (15) with the initial condition (16). The corresponding boundary conditions are as follows:(33)∂usy,t∂y|y=0=sinωt,us1,t=0fort>0.Dimensionless governing equations forτsy,t and σsy,t and the corresponding initial conditions are also given by equations (19) and (20) where the new constant α=λS2/μ.The solution of this new problem with initial and mixed boundary conditions can be determined following the same way as before. To avoid repetition, we here present the final results only. As usually, the dimensionless starting solutionsusy,t and τsy,t of such a motion that become steady in time can be presented under the forms as follows:(34)usy,t=uspy,t+usty,t,τsy,t=τspy,t+τsty,t,in which their steady-state (permanent or long time) and transient components are given by the next relations as follows:(35)uspy,t=y−1sinωt+2∑n=0∞bnsinωt+ωμn2cosωtan2+ω2cosμnyμn2,(36)τspy,t=sinωt−ωWecosωtωWe2+1,−2∑n=0∞bn+Weω2μn2sinωt+ωμn2−Webncosωtan2+ω2ωWe2+1sinμnyμn,(37)usty,t=2ω∑n=0∞an+r1ner2nt−an+r2ner1ntr2n−r1nan2+ω2cosμny,(38)τsty,t=ωexp−t/WeωWe2+1We−2∑n=0∞μn2−Webnan2+ω2sinμnyμn−2ω∑n=0∞an+r1nWer1n+1er2nt−an+r2nWer2n+1er1ntr2n−r1nan2+ω2Wer1n+1Wer2n+1μnsinμny+2ωexp−tWe∑n=0∞an+r1nWer1n+1−an+r2nWer2n+1r2n−r1nan2+ω2Wer1n+1Wer2n+1μnsinμny,where bn=anK+1−anWeω2.Direct computations show thatusy,t and τsy,t given by equation (34) satisfy both the corresponding governing equations and all imposed initial and boundary conditions. Sometime after the motion initiation, the fluid moves according to these solutions. After this time, when the transients disappear or can be neglected, the fluid motion is characterized by the steady-state solutions given by equations (35) and (36). It is worth pointing out that the steady-state components of usy,t and τsy,t can be also presented in the simpler forms as follows:(39)uspy,t=Imsinhy−1γγcoshγeiωt,τspy,t=Imcoshy−1γ1+iωWecoshγeiωt,where γ=K−Weω2+iω, i is the imaginary unit and Im denotes the imaginary part of that which follows. The equivalence of the steady-state solutions given by the equalities (35) and (36) with those from the relations (39) is graphically proved in Figures 2 and 3.Figure 2
Profiles of the steady-state componentuspy,t given by equalities (35) and (39) for ω=π/12,We=0.7,K=1 and 2, and three values of the time t.
(a)(b)Figure 3
Profiles of the steady-state componentτspy,t given by equalities (34) and (39) for ω=π/12,We=0.7,K=1 and 2, and three values of the time t.
(a)(b)The dimensionless steady-state and transient solutions corresponding to the motion of the incompressible Newtonian fluids induced by the lower plate that applies a oscillatory shear stress of form (6) to the fluid, namely,(40)uNspy,t=y−1sinωt+2∑n=0∞anK+ω2sinωt+ωμn2cosωtan2+ω2cosμnyμn2,(41)τNspy,t=sinωt−2∑n=0∞anK+ω2sinωt+ωμn2cosωtan2+ω2sinμnyμn,(42)uNsty,t=−2ω∑n=0∞cosμnyμn2+K2+ω2e−μn2+Kt,(43)τNsty,t=2ω∑n=0∞μnsinμnyμn2+K2+ω2e−μn2+Kt,are immediately obtained making We⟶0 in equations (35)–(38). As expected, the expressions of uNspy,t and uNsty,t given by equations (40) and (42), respectively, are also in accordance with the results obtained by Javaid et al. (see equalities (40) and (41) in [16]) where the corresponding boundary condition (8) has been taken with an opposite sign and a different normalization was considered.


## 3.1. Caseτ0,t=S1t−λ1−exp−t/λ

In order to determine solutions which are independent of the flow geometry, let us introduce the following nondimensional variables and functions:(14)y∗=yd,t∗=νd2t,u∗=μνd3S1u,τ∗=νd2S1τ,σ∗=νd2S1σ.Introducing the above nondimensional entities in equations (9)–(11) and giving up the star notation, the next mixed initial-boundary value problem(15)We∂2uy,t∂t2+∂uy,t∂t=∂2uy,t∂y2−Kuy,t;0<y<1,t>0,(16)uy,0=0,∂uy,t∂t|t=0=0for0≤y≤1,(17)∂uy,t∂y|y=0=t,u1,0=0ift>0,is obtained. In equation (15), the Weissenberg number We and the dimensionless porosity parameter K are defined by the equalities as follows:(18)We=λVd,K=ϕkd2,where V=ν/d is a characteristic velocity. The Weissenberg number We represents the ratio of the relaxation time λ and the characteristic time t0=d/V.The dimensionless forms of the ordinary differential equation (4) are(19)We∂τy,t∂t+τy,t=∂uy,t∂y,We∂σy,t∂t+σy,t=2ατy,t∂uy,t∂y;0<y<1,t>0,where α=λd2S1/μν. The corresponding initial conditions are(20)τy,0=0andσy,0=0;0≤y≤1.Multiplying equation (15) with cosμny, where μn=2n+1π/2, integrating the result from zero to one, and bearing in mind the initial and boundary conditions (16) and (17) and equalities (A.1) and (A.2) from Appendix, it results that the finite Fourier cosine transform uFnt of uy,t has to satisfy the ordinary differential equation as follows:(21)Wed2uFntdt2+duFntdt+μn2+KuFnt=−t;t>0,n=1,2,3...,with the initial conditions(22)uFn0=0,duFntdt|t=0=0;n=1,2,3...The solution of equation (21) with the initial conditions (22) is given by the relation as follows:(23)uFnt=1an−t+1an+an+r1ner2nt−an+r2ner1ntr2n−r1nan;n=1,2,3...,where an=μn2+K and r1n,2n=−1±1−4Wean/2We. On the basis of equality (A.1),it results that the dimensionless velocity field uy,t corresponding to this motion is given by(24)uy,t=2∑n=0∞−t+1an+an+r1ner2nt−an+r2ner1ntr2n−r1nancosμnyan;0<y<1,t>0,or equivalently (see the equality (A.3) from Appendix)(25)uy,t=y−1t+2tK∑n=0∞cosμnyanμn2+2∑n=0∞1+an+r1ner2nt−an+r2ner1ntr2n−r1ncosμnyan2.Direct computations clearly show thatuy,t given by equality (25) satisfies both the governing equation (15) and all imposed initial and boundary conditions. The dimensionless volume flux across a plane normal to the x-axis and per unit width of this plane is given by the relation as follows:(26)Q=Qt=−t2+2tK∑n=0∞−1nμn3μn2+K+2∑n=0∞1+an+r1ner2nt−an+r2ner1ntr2n−r1n−1nμn2+K2.Fort=0, as expected, Q becomes zero.In order to determine the dimensionless frictional force per unit area exerted by the fluid on the stationary plate, the corresponding shear stressτy,t has to be known. Replacing the expression of uy,t from equality (25) in (19) and solving the obtained equation with the initial condition (20), it results that τy,t is given by the following expression:(27)τy,t=t−We1−exp−tWe1−2K∑n=0∞sinμnyμnμn2+K−2∑n=0∞1+an+r1nWer1n+1er2nt−an+r2nWer2n+1er1ntr2n−r1nWer1n+1Wer2n+1μnsinμnyμn2+K2+2exp−tWe∑n=0∞1+an+r1nWer1n+1−an+r2nWer2n+1r2n−r1nWer1n+1Wer2n+1μnsinμnyμn2+K2.The motion whose solutions have been determined in this subsection is unsteady and remains unsteady. It is clear that at large enough values of the timet, the fluid motion can be described by the long time solutions:(28)uLty,t=y−1t+2tK∑n=0∞cosμnyμn2μn2+K+2∑n=0∞cosμnyμn2+K2,(29)τLty,t=t−We1−2K∑n=0∞sinμnyμnμn2+K−2∑n=0∞μnsinμnyμn2+K2.As expected, the dimensionless velocity and shear stress fieldsuNy,t and τNy,t corresponding to incompressible Newtonian fluids performing the same motion, namely, (30)uNy,t=y−1t+2tK∑n=0∞cosμnyμn2μn2+K+2∑n=0∞1−e−μn2+Ktcosμnyμn2+K2,(31)τNy,t=t−2tK∑n=0∞sinμnyμnμn2+K−2∑n=0∞1−e−μn2+Ktμnsinμnyμn2+K2,are immediately obtained making We⟶0 in equations (25) and (27). Of course, the last solutions are in agreement with the solutions obtained in equalities (29) and (31) in [16] where the boundary condition (8) has been taken with a changed sign. The corresponding volume flux QN can be immediately obtained making We=0 in the general expression of Q. In the absence of the porous effects, the corresponding solutions can be determined making K⟶0 into the above relations.From equalities (28) and (30), it clearly results that the long time velocity fields uLty,t and uNLty,t corresponding to the incompressible UCM and Newtonian fluids, respectively, are identical. Consequently, for large enough values of the time t, the dimensionless velocity field uLty,t corresponding to incompressible UCM fluids can be approximated with that of Newtonian fluids. Of course, bearing in mind known results from the existing literature, this is not a surprise. However, this property is not valid for the corresponding shear stress fields. The corresponding frictional forces per unit area exerted by the fluid on the upper plate can be immediately determined making y=1 in any one of the relations (27), (29), or (31).


## 3.2. Caseτ0,t=S2sinωt−λωcosωt−exp−t/λ/λω2+1

Introducing the next nondimensional variables, functions, and parameters such as(32)y∗=yd,t∗=νd2t,u∗=μdS2u,τ∗=τS2,σ∗=σS2,ω∗=d2νωin equality (9) and again dropping out the star notation, one obtains for the velocity field usy,t corresponding to this motion a dimensionless governing equation of the same form as (15) with the initial condition (16). The corresponding boundary conditions are as follows:(33)∂usy,t∂y|y=0=sinωt,us1,t=0fort>0.Dimensionless governing equations forτsy,t and σsy,t and the corresponding initial conditions are also given by equations (19) and (20) where the new constant α=λS2/μ.The solution of this new problem with initial and mixed boundary conditions can be determined following the same way as before. To avoid repetition, we here present the final results only. As usually, the dimensionless starting solutionsusy,t and τsy,t of such a motion that become steady in time can be presented under the forms as follows:(34)usy,t=uspy,t+usty,t,τsy,t=τspy,t+τsty,t,in which their steady-state (permanent or long time) and transient components are given by the next relations as follows:(35)uspy,t=y−1sinωt+2∑n=0∞bnsinωt+ωμn2cosωtan2+ω2cosμnyμn2,(36)τspy,t=sinωt−ωWecosωtωWe2+1,−2∑n=0∞bn+Weω2μn2sinωt+ωμn2−Webncosωtan2+ω2ωWe2+1sinμnyμn,(37)usty,t=2ω∑n=0∞an+r1ner2nt−an+r2ner1ntr2n−r1nan2+ω2cosμny,(38)τsty,t=ωexp−t/WeωWe2+1We−2∑n=0∞μn2−Webnan2+ω2sinμnyμn−2ω∑n=0∞an+r1nWer1n+1er2nt−an+r2nWer2n+1er1ntr2n−r1nan2+ω2Wer1n+1Wer2n+1μnsinμny+2ωexp−tWe∑n=0∞an+r1nWer1n+1−an+r2nWer2n+1r2n−r1nan2+ω2Wer1n+1Wer2n+1μnsinμny,where bn=anK+1−anWeω2.Direct computations show thatusy,t and τsy,t given by equation (34) satisfy both the corresponding governing equations and all imposed initial and boundary conditions. Sometime after the motion initiation, the fluid moves according to these solutions. After this time, when the transients disappear or can be neglected, the fluid motion is characterized by the steady-state solutions given by equations (35) and (36). It is worth pointing out that the steady-state components of usy,t and τsy,t can be also presented in the simpler forms as follows:(39)uspy,t=Imsinhy−1γγcoshγeiωt,τspy,t=Imcoshy−1γ1+iωWecoshγeiωt,where γ=K−Weω2+iω, i is the imaginary unit and Im denotes the imaginary part of that which follows. The equivalence of the steady-state solutions given by the equalities (35) and (36) with those from the relations (39) is graphically proved in Figures 2 and 3.Figure 2
Profiles of the steady-state componentuspy,t given by equalities (35) and (39) for ω=π/12,We=0.7,K=1 and 2, and three values of the time t.
(a)(b)Figure 3
Profiles of the steady-state componentτspy,t given by equalities (34) and (39) for ω=π/12,We=0.7,K=1 and 2, and three values of the time t.
(a)(b)The dimensionless steady-state and transient solutions corresponding to the motion of the incompressible Newtonian fluids induced by the lower plate that applies a oscillatory shear stress of form (6) to the fluid, namely,(40)uNspy,t=y−1sinωt+2∑n=0∞anK+ω2sinωt+ωμn2cosωtan2+ω2cosμnyμn2,(41)τNspy,t=sinωt−2∑n=0∞anK+ω2sinωt+ωμn2cosωtan2+ω2sinμnyμn,(42)uNsty,t=−2ω∑n=0∞cosμnyμn2+K2+ω2e−μn2+Kt,(43)τNsty,t=2ω∑n=0∞μnsinμnyμn2+K2+ω2e−μn2+Kt,are immediately obtained making We⟶0 in equations (35)–(38). As expected, the expressions of uNspy,t and uNsty,t given by equations (40) and (42), respectively, are also in accordance with the results obtained by Javaid et al. (see equalities (40) and (41) in [16]) where the corresponding boundary condition (8) has been taken with an opposite sign and a different normalization was considered.


## 4. Some Numerical Results and Discussion

Exact solutions for two dimensionless mixed initial-boundary value problems corresponding to unsteady motions of incompressible UCM fluids through a porous plate channel have been established in a simple way using the finite Fourier cosine transform only. Their limiting expressions, when the relaxation timeλ and therefore the Weissenberg number We tends to zero, correspond to motions of the incompressible Newtonian fluids induced by the lower plate that applies ramp type or oscillating shear stresses to the fluid. The steady-state solutions uspy,t and τspy,t corresponding to the second motion which becomes steady in time are presented in different forms whose equivalence is graphically proved in Figures 2 and 3. This proof, as well as the fact that known solutions from the existing literature for the incompressible Newtonian fluids are recovered as limiting cases of the present results, could be an evidence of the correctness of present results. The presentation of the starting solutions of a given motion as a sum of its steady-state and transient components is important for the experimentalists who want to eliminate the transients from their experiments.To get some physical insight of present results, the influence of the Weissenberg number We and the porosity parameterK on the fluid motion has been brought to light in Figures 4 and 5. The required time to reach the steady-state for the motion which becomes steady in time is graphically determined in Figures 6 and 7 for two distinct values of We and K, respectively. This is the time after which the diagrams of the starting solution usy,t superpose over those of its steady-state component uspy,t. In practice, as we previously mentioned, this time is important for those who want to eliminate the transients from their experiments. The time variations of the midplane steady-state velocity and shear stress fields are presented in Figures 8 and 9 for K=0.5 and 1 and different values of We.Figure 4
Variations of the velocity fieldsuy,t and uNy,t given by equations (25) and (30), respectively, for K=1,t=2 and 3, and three values of the Weissenberg number We.
(a)(b)Figure 5
Variation of the velocity fielduy,t given by equality (25) for We=0.7,t=2 and 3, and three values of the porosity parameter K.
(a)(b)Figure 6
Necessary time to reach the steady-state for the motion which becomes steady in time forω=π/12,K=1, and two values of the Weissenberg number We.
(a)(b)Figure 7
Necessary time to reach the steady-state for the motion which becomes steady in time forω=π/12,We=1.5, and two values of the porosity parameter K.
(a)(b)Figure 8
Time variations of the midplane velocitiesusp0.5,t and uNsp0.5,t for ω=π/12,K=1 and 2, and three values of the Weissenberg number We.
(a)(b)Figure 9
Time variations of the midplane shear stressesτsp0.5,t and τNsp0.5,t for ω=π/12,K=0.5 and 1, and three values of the Weissenberg number We.
(a)(b)In Figure4, for comparison, the diagrams of the velocity fields uy,t and uNy,t given by equalities (25) and (30), respectively, are together presented at two distinct values of the time t for decreasing values of We. The profiles of the starting solution uy,t are also presented in Figure 5 for three decreasing values of K. In all cases, the fluid velocity in absolute value smoothly decreases from maximum values on the lower plate to the zero value on the stationary plate. As expected, in absolute value, it is an increasing function with respect to the time t and diminishes for increasing values of K. Consequently, as expected, in the presence of a porous medium, the fluid motion becomes more difficult. Moreover, as it results from Figure 4, the fluid velocity uy,t in absolute value is a decreasing function with regard to the Weissenberg number We and converges to the Newtonian solution uNy,t if We⟶0. This behavior of the motion of the Maxwell fluid can be explained by the fact that, as it was proved by Poole [26], the Weissenberg number represents the ratio of elastic forces to viscous forces. Consequently, at the same elastic properties of the fluid, an increase in We means a diminution of viscous forces and therefore an increase in the fluid velocity.Time convergence of the starting solutionusy,t to its steady-state component uspy,t is shown in Figures 6 and 7 for distinct values of We and K. From these figures, it also results that the required time to reach the steady-state for this motion that becomes permanent in time is an increasing function with regard to the Weissenberg number We and diminishes for increasing values of the porosity parameter K. This means that the steady-state is rather obtained for the oscillatory motion of the incompressible Newtonian fluids induced by sine oscillations of the shear stress on the boundary as compared with incompressible UCM fluids whose motion is generated by a shear stress of form (5) on the boundary. In the same time, it is clearly seen from Figure 7 that the presence of the porous medium hastens the appearance of the steady-state. The boundary condition on the upper plate is clearly satisfied.The time variations of the midplane dimensionless steady-state velocity and shear stress fieldsusp0.5,t, τsp0.5,t and uNsp0.5,t, τNsp0.5,t corresponding to incompressible UCM and Newtonian fluids, respectively, are together presented in Figures 8 and 9 for K=0.5, K=1, and three distinct values of the Weissenberg number We. In all cases, the convergence of the non-Newtonian solutions usp0.5,t and τsp0.5,t to the corresponding Newtonian solutions if We⟶0, as well as the oscillating specific features of the fluid motion, is clearly visualized. The amplitude of the oscillations, as expected, diminishes for increasing values of K both for velocity and shear stress. In addition, the values of the velocity usp0.5,t and those of the corresponding shear stress τsp0.5,t have opposite signs at each time t.


## 5. Conclusions

Two mixed initial-boundary value problems characterizing unsteady motions of the UCM fluids between infinite parallel plates are analytically studied. Closed-form expressions are established for the dimensionless velocity and shear stress fields using the finite Fourier cosine transform. The influence of essential physical parameters on the fluid behavior was graphically investigated, and the obtained results can be such summarized:(i)
Analytical solutions for two mixed initial-boundary value problems corresponding to nonsteady motions of UCM fluids through a porous plate channel are determined.(ii)
The necessary time to touch the steady-state is graphically provided. It is an increasing function with respect to We and diminishes for increasing values of the parameterK.(iii)
Presence of porous medium hastens the appearance of the steady-state of the motion.(iv)
The amplitude of the oscillations corresponding to the steady-state solutions wanes in the presence of a porous medium both for the fluid velocity and the adequate shear stress.(v)
Solutions corresponding to movements of Newtonian fluids induced by ramp type or oscillatory shear stresses on the boundary are acquired as limiting cases of the present results.



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*Source: 5539007-2021-04-26.xml*