Unsteady Unidirectional MHD Flow of Voigt Fluids Moving between Two Parallel Surfaces for Variable Volume Flow Rates

Abstract

The velocity profile and pressure gradient of an unsteady state unidirectional MHD flow of Voigt fluids moving between two parallel surfaces under magnetic field effects are solved by the Laplace transform method. The flow motion between parallel surfaces is induced by a prescribed inlet volume flow rate that varies with time. Four cases of different inlet volume flow rates are considered in this study including (1) constant acceleration piston motion, (2) suddenly started flow, (3) linear acceleration piston motion, and (4) oscillatory piston motion. The solution for each case is elaborately derived, and the results of associated velocity profile and pressure gradients are presented in analytical forms.

1. Introduction

Magnetohydrodynamics (MHD) is an academic discipline, which studies the dynamic behaviors of the interaction between magnetic fields and electrically conducting fluids. Examples of such fluids are numerous including plasmas, liquid metals, and salt water or electrolytes. The MHD flow is encountered in a variety of applications such as MHD power generators, MHD pumps, MHD accelerators, and MHD flowmeters, and it can also be expanded into various industrial uses.

During the past decades, a great deal of papers in literatures used a combination of Navier-Stokes equations and Maxwell's equations to describe the MHD flow of the Newtonian and electrically conducting fluid. Sayed-Ahmed and Attia [1] examined the effect of the Hall term and the variable viscosity on the velocity and temperature fields of the MHD flow. Attia [2] studied the unsteady Couette flow and heat transfer of a dusty conducting fluid between two parallel plates with variable viscosity and electrical conductivity. Osalusi et al. [3] solved unsteady MHD and slip flow over a porous rotating disk in the presence of Hall and ion-slip currents by using a shooting method.

However, the Newtonian fluid is the simplest to be solved and its application is very limited. In practice, many complex fluids such as blood, suspension fluids, certain oils, greases and polymer solution, elastomers, and many emulsions have been treated as non-Newtonian fluids.

From the literature, the non-Newtonian fluids are principally classified on the basis of their behavior in shear. A fluid with a linear relationship between the shear stress and the shear rate, giving rise to a constant viscosity, is always characterized to be a Newtonian fluid. Based on the knowledge of solutions to Newtonian fluid, the different fluids can be extended, such as Maxwell fluids, Voigt fluids, Oldroyd-B fluids, Rivlin-Ericksen fluids, and power-law fluids. In this study, we investigate the flow characteristics of the MHD flow of Voigt fluids.

The exact solutions for laminar flow in a duct with a given pressure gradient varying with time are well known. For example, Szymanski [4] gave solutions for impulsively imposed pressure gradient. For more complex cases of the Maxwell fluid, Rahaman and Ramkissoon [5] provided solutions for a pressure gradient varying exponentially with time, sinusoidal pulsating pressure gradient and constant pressure gradient. Hayat et al. [6] solved for exact solution to some simple flows of an Oldroyd-B fluid between two parallel surfaces with and without pressure gradient. Some researchers studied the flow motion caused by the movement of a boundary. Bandelli and Rajagopal [7] solved for various start-up flows of second grade fluids in domains with one finite dimension by an integral transform method. Huang and Liu [8] analytically investigated the character of viscoelastic fluids in a double-gap concentric cylinder rheometer.

In general for more realistic applications, the volume flow rates are given as the inlet condition instead of the pressure gradient. For a power law fluid, J. P. Pascal and H. Pascal [9] solved this problem by similarity transformation method. Das and Arakeri [10] gave an analytical solution for various transient volume flow rates for a Newtonian fluid, which complemented with earlier experimental work [11]. Chen et al. [12–16] extended Das and Arakeri’s work by considering various non-Newtonian fluids. Hayat et al. considered the unsteady flow of an incompressible second-grade fluid in a circular duct with a given volume flow rate variation [17]. And further, Hayat et al. presented a lot of researches about the MHD flows of non-Newtonian fluids [18–36].

Based upon previous studies, we, therefore, further investigate in this paper the flow characteristics of Voigt fluids under magnetic field effects.

2. Mathematical Formulations

The unidirectional rheological equation of state for a Voigt fluid in 𝑥-direction is given by Lee and Tsai [37] 𝑇^→_𝑖𝑗=−𝑝𝛿_𝑖𝑗𝜏+𝜏_𝑖𝑗,𝑖=𝑥,𝑦,𝑧,𝑗=𝑥,(2.1)_𝑦𝑥=𝐺𝜈+𝜇𝜈̇,(2.2) where 𝑇_𝑖𝑗 is the total stress, subscript 𝑖 denotes the normal direction of 𝑖-plane, subscript 𝑗 denotes the stress acting direction, 𝑝 is the static fluid pressure (𝑝=𝑝(𝑥,𝑦,𝑧)), 𝛿_𝑖𝑗 is the Kronecker delta, 𝜏_𝑖𝑗 is the shear stress, 𝐺 is the rigidity modulus, 𝜈 is the shear strain, 𝜈̇ is the rate of shear strain, and 𝜇 is the viscosity coefficient. Here 𝐺, 𝜇 are the material properties and are assumed to be constant. When 𝐺=0, (2.2) reduces to that of Newtonian fluid.

The problem of the unsteady flow of incompressible Voigt fluid between the parallel surfaces is considered. The dynamic equation is ∇⋅𝑇^→+𝜌^→𝑏=𝜌𝑑^→𝑉𝑑𝑡.(2.3) In the above equation, 𝑇^→ denotes the total stress tensor, 𝜌 the fluid density, 𝑉^→ the velocity vector, ^→𝑏 the body force field, and ∇ the divergence operator.

The continuity equation is ∇⋅𝑉^→=0.(2.4) Using the Cartesian coordinate system (𝑥,𝑦,𝑧), the 𝑥-axis is taken as the centerline direction between these two parallel surfaces, 𝑦 is the coordinate normal to the plate, 𝑧 is the coordinate normal to 𝑥 and 𝑦, respectively, and the velocity field is assumed in the form 𝑉^→=𝑢(𝑦,𝑡)^→𝑖,(2.5) where 𝑢 is the velocity in the 𝑥-coordinate direction and ^→𝑖 is the unit vector in the 𝑥-coordinate direction. This effectively assumes that the flow is fully developed at all points in time.

Substituting of (2.5) into (2.4) shows that the continuity equation automatically satisfied the result of substituting in (2.1) and (2.3). So we have the following scalar equation: 𝜕𝑝𝜕𝑥=𝜕𝜕𝜏𝑦^𝑦𝑥−𝜌𝜕𝜕𝑢𝑡−𝜎𝐵⁰²𝑢,(2.6) where 𝐵₀ is the electromagnetic field, subscript 𝑦 denotes the plane normal to 𝑦 direction, 𝑥 the direction along the shear stress, and 𝜕𝑝𝜕𝑦=𝜕𝜕𝑧𝑝=0,(2.7) where the body force is incorporated into the term of pressure gradient.

Equations (2.6) and (2.7) imply that the pressure gradient is a function of time only.

Solving (2.2) subject to 𝜏_𝑦𝑥=0 and 𝜈̇=𝜕𝑢/𝜕𝑦=0 as 𝑡=0, the strain function is obtained 𝜈(𝑡)=1𝜇𝑒^{−(𝐺/𝜇)𝑡}^𝑡0𝜏_𝑦𝑥𝑒^{(𝐺/𝜇)𝑡′}𝑑𝑡^,(2.8) where 𝑡′ is the integration dummy variable.

Equations (2.6) and (2.8) are our governing equations describing the Voigt fluid flowing between the parallel surfaces.

3. Methodology of Solution

Since the governing equation with boundary conditions and initial condition are known, the problem is well posed. In general, it is not an easy question to solve this kind of equation by the method of separation of variables and eigenfunctions expansion. In this paper, the Laplace transform method is used to reduce the two variables into a single variable. This procedure greatly reduces the difficulties of treating these partial differential [9] and integral equations [11].

The governing equation of motion in 𝑥-direction and the strain function are 𝜕𝑝𝜕𝑥=𝜕𝜕𝜏𝑦^𝑦𝑥−𝜌𝜕𝜕𝑢𝑡−𝜎𝐵⁰²𝜈(𝑡)=1𝑢,(3.1)𝜇𝑒^{−(𝐺/𝜇)𝑡}^𝑡0𝜏_𝑦𝑥𝑒^{(𝐺/𝜇)𝑡′}𝑑𝑡^.(3.2) As these two surfaces are 2ℎ apart, the boundary conditions are 𝜕𝑢𝑢((ℎ0,,𝑡𝑡))=0,𝜕𝑦=0.(3.3) The initial condition is related to the inlet volume flow rate by ^ℎ−ℎ𝑢(𝑦,𝑡)𝑑𝑦=𝑢_𝑝(𝑡)2ℎ=𝑄(𝑡),(3.4) where 𝑢_𝑝(𝑡) is the given average inlet velocity and 𝑄(𝑡) is the given inlet volume flow rate.

The above governing equation, boundary conditions, and initial condition are prescribed and can be solved by the following calculation of Laplace transform.

Differentiating (3.2) with respect to time and taking Laplace transform, then we have 𝜏̂_𝑦𝑥(𝑦,𝑠)=𝜇𝑠+𝐺𝑠𝜕𝑢̂𝜕(𝑦𝑦,𝑠).(3.5)

Taking the Laplace transform of (3.1) and substituting (3.5) into it, we have the governing equation 𝜕²𝑢̂(𝑦,𝑠)𝜕𝑦²−𝜌𝑠²+𝜎𝐵₀₂𝑠𝜇𝑠+𝐺𝑢̂(𝑦,𝑠)=𝜇𝑠𝑠+𝐺𝜕𝑝̂𝜕(𝑥𝑥,𝑠).(3.6)

Considering the governing equation as an ordinary differential equation (with respect to 𝑦) and boundary conditions 𝑑𝑢𝑢̂(̂ℎ(0,,𝑠𝑠))=0,(3.7)𝑑𝑦=0,(3.8) and initial condition ^ℎ−ℎ𝑢̂(𝑦,𝑠)𝑑𝑦=𝑢_𝑝̂(𝑠)2ℎ,(3.9) the general solution of (3.6) is 𝑢̂(𝑦,𝑠)=𝐶₁sinh𝑚𝑦+𝐶₂cosh𝑚𝑦+Ψ_𝑝,(3.10) where Ψ_𝑝 is the assumed particular solution and 𝑚=(𝜌𝑠²+𝜎𝐵₀₂𝑠)/(𝜇𝑠+𝐺).

The boundary conditions (3.7) and (3.8) are used to solve the two arbitrary coefficients 𝐶₁ and 𝐶₂. Substituting 𝐶₁ and 𝐶₂ into (3.10) gives 𝑢̂(𝑦,𝑠)=Ψ_𝑝1−ccoosshh𝑚𝑚ℎ𝑦.(3.11) Substituting (3.11) into the initial condition of (3.9), Ψ_𝑝 is readily obtained as Ψ_𝑝^ℎ−ℎ1−ccoosshh𝑚𝑚ℎ𝑦𝑑𝑦=𝑢^𝑝̂(𝑠)2ℎ(3.12) or Ψ_𝑝=𝑢^𝑝̂(𝑠)(1−sinh𝑚ℎ/𝑚ℎcosh𝑚ℎ).(3.13) Substituting Ψ_𝑝 into (3.11) gives 𝑢̂(𝑦,𝑠)=𝑢^𝑝̂(𝑠)(cosh𝑚ℎ−cosh𝑚𝑦)(cosh𝑚ℎ−sinh𝑚ℎ/𝑚ℎ)(3.14) or 𝑢̂(𝑦,𝑠)=𝑢_𝑝̂(𝑠)Ω(𝑦,𝑠),(3.15) where Ω(𝑦,𝑠)=(cosh𝑚ℎ−cosh𝑚𝑦)(cosh𝑚ℎ−sinh𝑚ℎ/𝑚ℎ).(3.16) Taking the inverse Laplace transform, the velocity profile is 𝑢(𝑦,𝑡)=12𝜋𝑖^{𝛾+𝑖∞𝛾−𝑖∞}𝑢_𝑝̂(𝑠)Ω(𝑦,𝑠)𝑒^𝑠𝑡𝑑𝑠.(3.17) Furthermore, the pressure gradient is found by substituting (3.11) into (3.6) to give 𝜕𝑝̂(𝑥,𝑠)𝜕𝑥=−𝜌𝑠+𝜎𝐵⁰²Ψ_𝑝(3.18) or 𝜕𝑝̂(𝑥,𝑠)𝜕𝑥=−𝜌𝑠+𝜎𝐵⁰²𝑢^𝑝̂(𝑠)cosh𝑚ℎ(cosh𝑚ℎ−sinh𝑚ℎ/𝑚ℎ).(3.19) Using the inverse transform formula, the pressure gradient distribution can also be obtained.

4. Illustration of Examples

Hereafter, we will solve the cases proposed by Das and Arakeri [10] with the Voigt fluid to understand the different flow characteristics between these two fluids under the same condition.

For the first case, the piston velocity 𝑢_𝑝(𝑡) moves with a constant acceleration and for the second one, the piston starts suddenly from rest and then maintains this velocity. These two solutions are used to assess the trapezoidal motion of the piston, namely, the piston has three stages: constant acceleration of piston starting from rest, a period of constant velocity, and a constant deceleration of the piston to a stop. Finally, the oscillatory piston motion is also considered.

4.1. Constant Acceleration Piston Motion

The piston motion of constant acceleration can be described by the following equation: 𝑢_𝑝(𝑡)=𝑎_𝑝𝑡=𝑈^𝑝𝑡₀𝑡,(4.1) where 𝑎_𝑝 is the constant acceleration, 𝑈_𝑝 is the final velocity after acceleration, and 𝑡₀ is the time period of acceleration.

Taking the Laplace transform of (4.1), 𝑢_𝑝̂(𝑠)=𝑈^𝑝𝑡₀𝑠².(4.2) From (3.17) and (4.2), the velocity profile is 𝑢(𝑦,𝑡)=12𝜋𝑖^{𝑟+𝑖∞𝑟−𝑖∞}𝑈_𝑝𝑡₀𝑠²(cosh𝑚ℎ−cosh𝑚𝑦)(cosh𝑚ℎ−sinh𝑚ℎ/𝑚ℎ)𝑒^𝑠𝑡𝑑𝑠.(4.3) From the above expression, the integration is determined using complex variable theory, as discussed by Arpaci [38]. It is easily observed that 𝑠=0 is a pole of order 2.

Therefore, the residue at 𝑠=0 is Res(0)=𝑈_𝑝23𝑡𝑡₀1−ℎ𝑦².(4.4) The other singular points are the roots of following transcendental equation: 𝑚ℎcosh𝑚ℎ−sinh𝑚ℎ=0.(4.5) Setting 𝑚=𝑖𝛼, we have 𝛼ℎcos𝛼ℎ−sin𝛼ℎ=0(4.6) or tan𝛼ℎ=𝛼ℎ.(4.6b) If 𝛼_𝑛, 𝑛=1,2,3,...,∞, are zeros of (4.6), then 𝑠_1𝑛=−𝜎𝐵⁰²+𝛼^2𝑛𝜇+𝜎𝐵₀₂+𝛼^2𝑛𝜇²−4𝜌𝛼^2𝑛𝐺𝑠2𝜌_2𝑛,=−𝜎𝐵⁰²+𝛼^2𝑛𝜇−𝜎𝐵₀₂+𝛼^2𝑛𝜇²−4𝜌𝛼^2𝑛𝐺2𝜌,(4.7)𝑛=1,2,3,...,∞, are these poles. These are simple poles, and residues at all of these poles can be obtained as Res𝑠_1𝑛=𝑈^𝑝𝑡₀𝑒^{𝑠1𝑛𝑡}Res𝑠_2𝑛2𝑠_1𝑛𝑄+𝑠_21𝑛𝑄′𝑠_1𝑛,=𝑈𝑡^𝑝₀𝑒^{𝑠2𝑛𝑡}2𝑠_2𝑛𝑄+𝑠_22𝑛𝑄′𝑠_2𝑛,(4.8) where 𝑄𝑚=′𝛼𝑠_𝑛ℎ_𝑖𝑛cos𝛼_𝑛ℎ−sin𝛼_𝑛ℎ,𝑄′𝑠_𝑖𝑛=𝛼_𝑛𝑚′𝑠_𝑖𝑛ℎ²sin𝛼_𝑛ℎ,𝑖=1,2,=𝜕𝑚𝑠^𝑖𝑛𝜕𝑠=12𝜇𝜌𝑠^2𝑖𝑛+2𝐺𝜌𝑠_𝑖𝑛+𝐺𝜎𝐵₀₂𝜌𝑠_2𝑖𝑛+𝜎𝐵₀₂𝑠_𝑖𝑛^0.5𝜇𝑠_𝑖𝑛+𝐺^1.5,𝑖=1,2.(4.9)

Adding Res(0), Res(𝑠_1𝑛), and Res(𝑠_2𝑛), a complete solution for constant acceleration case is obtained as 𝑢(𝑦,𝑡)𝑡₀𝑈_𝑝=3𝑡21−ℎ𝑦²+^∞_𝑛=12𝑠_1𝑛𝑄+𝑒𝑠^{𝑠1𝑛𝑡}_21𝑛𝑄′𝑠_1𝑛+2𝑠_2𝑛𝑄+𝑒𝑠^{𝑠2𝑛𝑡}_22𝑛𝑄′𝑠_2𝑛𝑅(𝑦),(4.10) where 𝑅(𝑦)=𝛼_𝑛ℎ(cos𝛼_𝑛ℎ−cos𝛼_𝑛𝑦) and 𝑄,𝑄′(𝑠_1𝑛), 𝑄′(𝑠_2𝑛) are defined in (4.9).

The first term on the right-hand side of (4.10) represents the steady state velocity and the second term, the transient response of the flow to an abrupt change either in the boundary conditions, body forces, pressure gradient, or other external driving force.

Equation (3.19) is used to determine the pressure gradient in this flow field and follows the same procedure for solving velocity profile Res(0)=−𝜌𝑈^𝑝𝑡₀32𝑡2𝜌+𝜎𝐵⁰²Res𝑠_1𝑛𝑡,=−𝜌𝑡𝑈^𝑝₀𝜌𝑠_1𝑛+𝜎𝐵₀₂𝛼_𝑛ℎcos𝛼_𝑛ℎ2𝑠_1𝑛𝑄+𝑠_21𝑛𝑄′𝑠_1𝑛𝑒^{𝑠1𝑛𝑡}Res𝑠_2𝑛,=−𝜌𝑡𝑈^𝑝₀𝜌𝑠_2𝑛+𝜎𝐵₀₂𝛼_𝑛ℎcos𝛼_𝑛ℎ2𝑠_2𝑛𝑄+𝑠_22𝑛𝑄′𝑠_1𝑛𝑒^{𝑠2𝑛𝑡}.(4.11) Therefore, the pressure gradient is 𝜕𝑝(𝑥,𝑡)𝜕𝑥=−𝜌𝑡𝑈^𝑝₀32𝑡2𝜌+𝜎𝐵⁰²𝑡+^∞_𝑛=1𝜌𝑠^1𝑛+𝜎𝐵₀₂𝛼_𝑛ℎcos𝛼_𝑛ℎ2𝑠_1𝑛𝑄+𝑠_21𝑛𝑄^{(𝑠1𝑛)}𝑒^{𝑠1𝑛𝑡}+𝜌𝑠^2𝑛+𝜎𝐵₀₂𝛼_𝑛ℎcos𝛼_𝑛ℎ2𝑠_2𝑛𝑄+𝑠_22𝑛𝑄^{(𝑠2𝑛)}𝑒^{𝑠2𝑛𝑡}.(4.12)

𝑄, 𝑄′(𝑠_1𝑛), 𝑄′(𝑠_2𝑛) are defined in (4.9).

4.2. Suddenly Started Flow

For a suddenly started flow between the parallel surfaces, 𝑢_𝑝=𝑈0,for𝑡≤0,_𝑝,for𝑡>0,(4.13) where 𝑈_𝑝 is the constant velocity.

In which case, the velocity profile is 𝑢(𝑦,𝑡)𝑈_𝑝=321−ℎ𝑦²+^∞_𝑛=1𝑄+𝑠𝑒_1𝑛𝑄^{𝑠1𝑛𝑡}′𝑠_1𝑛+𝑄+𝑠𝑒_1𝑛𝑄^{𝑠2𝑛𝑡}′𝑠_1𝑛𝑅(𝑦),(4.14) where 𝑅(𝑦)=𝛼_𝑛ℎ(cos𝛼_𝑛ℎ−cos𝛼_𝑛𝑦), 𝑄, 𝑄′(𝑠_1𝑛), 𝑄′(𝑠_2𝑛) are defined in (4.9), and the pressure gradient is 𝜕𝑝(𝑥,𝑡)𝜕𝑥=−𝜌𝑈^𝑝32𝜎𝐵⁰²+^∞_𝑛=1𝜌𝑠^1𝑛+𝜎𝐵₀₂𝛼_𝑛ℎcos𝛼_𝑛ℎ𝑄+𝑠_1𝑛𝑄^{(𝑠1𝑛)}𝑒^{𝑠1𝑛𝑡}+𝜌𝑠^2𝑛+𝜎𝐵₀₂𝛼_𝑛ℎcos𝛼_𝑛ℎ𝑄+𝑠_2𝑛𝑄^{(𝑠2𝑛)}𝑒^{𝑠2𝑛𝑡}.(4.15)

4.3. Linear Acceleration Piston Motion

The piston motion of linear acceleration can be described by the following equation: 𝑢_𝑝(𝑡)=𝑎_𝑝𝑡²=𝑈^𝑝𝑡₀𝑡²,(4.16) where 𝑎_𝑝 is the constant acceleration, 𝑈_𝑝 is the final velocity after acceleration, and 𝑡₀ is the time period of acceleration.

In which case, the velocity profile is 𝑢(𝑦,𝑡)𝑡₀𝑈_𝑝=3𝑡²1−ℎ𝑦²+2^∞_𝑛=13𝑠_21𝑛𝑄+𝑒𝑠^{𝑠1𝑛𝑡}_31𝑛𝑄′𝑠_1𝑛+3𝑠_22𝑛𝑄+𝑒𝑠^{𝑠2𝑛𝑡}_32𝑛𝑄′𝑠_2𝑛𝑅(𝑦),(4.17) where 𝑅(𝑦)=𝛼_𝑛ℎ(cos𝛼_𝑛ℎ−cos𝛼_𝑛𝑦), 𝑄, 𝑄′(𝑠_1𝑛), 𝑄′(𝑠_2𝑛) are defined in (4.9), and the pressure gradient is 𝜕𝑝(𝑥,𝑡)𝜕𝑥=−2𝑡₀𝜌𝑈_𝑝23𝑡2𝜌+𝜎𝐵⁰²𝑡+2^∞_𝑛=1𝜌𝑠^1𝑛+𝜎𝐵₀₂𝛼_𝑛ℎcos𝛼_𝑛ℎ3𝑠_21𝑛𝑄+𝑠_31𝑛𝑄^{(𝑠1𝑛)}𝑒^{𝑠1𝑛𝑡}+𝜌𝑠^2𝑛+𝜎𝐵₀₂𝛼_𝑛ℎcos𝛼_𝑛ℎ3𝑠_22𝑛𝑄+𝑠_32𝑛𝑄^{(𝑠2𝑛)}𝑒^{𝑠2𝑛𝑡}.(4.18)

4.4. Oscillatory Piston Motion

The oscillating piston motion starting from rest is considered. The piston motion is described as 𝑢_𝑝=𝑈0,for𝑡≤0,₀sin(𝜔𝑡),for𝑡>0.(4.19) Taking the Laplace transform of (4.19), we have 𝑢_𝑝̂(𝑠)=𝑈⁰𝜔𝑠²+𝜔²𝑠>0.(4.20) Substituting (4.20) into (3.17) to find the velocity profile, the poles are simple poles at 𝑠=±𝑖𝜔 and the roots of 𝛼ℎcos𝛼ℎ−sin𝛼ℎ=0. The solution to the velocity profile is 𝑢(𝑦,𝑡)𝑈₀=𝑖2𝑒^{−𝑖𝜔𝑡}+Ω(𝑦,−𝑖𝜔)−𝑒^𝑖𝜔𝑡Ω(𝑦,𝑖𝜔)_∞_𝑛=12𝑠_1𝑛𝑄+𝑒𝑠^{𝑠1𝑛𝑡}_21𝑛𝑄′𝑠_1𝑛+2𝑠_2𝑛𝑄+𝑒𝑠^{𝑠2𝑛𝑡}_22𝑛𝑄′𝑠_2𝑛𝑅(𝑦),(4.21) where 𝑅(𝑦)=𝛼_𝑛ℎ(cos𝛼_𝑛ℎ−cos𝛼_𝑛𝑦), 𝑄, 𝑄′(𝑠_1𝑛), 𝑄′(𝑠_2𝑛) are defined in (4.9), Ω(𝑦,𝑠) is defined by (3.16), and the pressure gradient is obtained as 𝜕𝑝(𝑥,𝑡)𝜕𝑥=−𝜌𝑈2⁰𝑖𝜌𝜔+𝜎𝐵⁰²𝑒^𝑖𝜔𝑡+Γ(𝑖𝜔)+−𝑖𝜔𝜌+𝜎𝐵₀₂𝑒^{−𝑖𝑖𝜔𝑡}Γ(−𝑖𝜛)_∞_𝑛=1𝜌𝑠^1𝑛+𝜎𝐵₀₂𝛼_𝑛ℎcos𝛼_𝑛ℎ2𝑠_1𝑛𝑄+𝑠_21𝑛+𝜔²𝑄′𝑠_1𝑛𝑒^{𝑠1𝑛𝑡}+𝜌𝑠^2𝑛+𝜎𝐵₀₂𝛼_𝑛ℎcos𝛼_𝑛ℎ2𝑠_2𝑛𝑄+𝑠_22𝑛+𝜔²𝑄′𝑠_1𝑛𝑒^{𝑠2𝑛𝑡},(4.22) where 𝑄, 𝑄′(𝑠_1𝑛), 𝑄′(𝑠_2𝑛) are defined in (4.9), and Γ(𝑠)=cosh𝑚ℎ(cosh𝑚ℎ−sinh𝑚ℎ/𝑚ℎ),𝑚=𝜌𝑠²+𝜎𝐵₀₂𝑠𝜇𝑠+𝐺.(4.23)

5. Conclusions

In this paper, the analytical solutions of unsteady unidirectional MHD flow of Voigt fluids under magnetic field effects for different piston motion that provide different volume flow rates are derived and solved by Laplace transform technique. The results are presented in analytical forms.

The pressure gradient for each flow condition is thus being derived from the known function of inlet volume flow rate by using the same method. It is interested to note that for fully developed flows the relaxation time only appears as the motion is unsteady.