ABSTRACT

In this paper, we presents some new exact solutions corresponding to three unsteady flow problems of a generalized Jeffrey fluid produced by a flat plate between two side walls perpendicular to the plate. The fractional calculus approach is used in the governing equations. The exact solutions are established by means of the Fourier sine transform and N-transform. The series solutions of velocity field and associated shear stress in terms of Fox H-function, satisfying all imposed initial and boundary conditions, have been obtained. The similar solutions for ordinary Jeffrey fluid, performing the same motion, appear as limiting case of the solutions are also obtained. Also, the obtained results are analyzed graphically through various pertinent parameters.

Keywords:

Generalized Jeffrey Fluid, Fractional Derivatives, Fox H-Functions, N-Transform

1. Introduction

Impressive advancement has been made in examining streams of non-Newtonian fluids in the most recent couple of decades. Non-Newtonian fluids have both the properties of elasticity as well as viscosity. The examples of such fluids are very large but we give some of them like honey, toothpaste, ketchup, oils and paints etc. These fluids are widely used in our life and have many interesting applications. It has been proven by many researchers that such kinds of fluids are not only important to academia but also to industry such as polymer processing and making of food and paper.

As we know that Newtonian fluids are modeled by a single equation, the flows of non-Newtonian fluids cannot be explained by a single constitutive model. In general the rheological properties of fluids are specified by their so-called constitutive equations. Exact recent solutions for constitutive equations of viscoelastic fluids are given by Rajagopal and Bhatnagar [1] , Tan and Masuoka [2] [3] , Fetecau and C. Fetecau [4] [5] , Khadrawi et al. [6] , and Chen et al. [7] etc. Amongst non-Newtonian fluids the Jeffrey model is considered to be one of the simplest model which best explains the rheological effects of viscoelastic fluids. The Jeffrey model is a relatively simple linear model using the time derivatives instead of convected derivatives.

Recently, the fractional derivative [8] [9] approach has proved to be an important tool for considering behaviors of such types of fluids. Many researchers investigated different problems using the fractional derivative technique for such fluids. In their work, integer order time derivatives in the constitutive models for generalized Jeffrey fluids were replaced by the Riemann-Liouville fractional derivatives. A lot of work has been done on fractional derivatives during the last few years. Bagley [10] proved that fractional derivative models of viscoelastic type fluids were in harmony with the molecular theory and attains the fractional differential equation of order 1/2. Friedrich [11] developed the fractional derivative method into rheology to investigate various problems. Li and Jiang [12] employ the fractional calculus to examine the behavior of sesbania gum and Xanthan gum in their experiments and attain adequate results. Moreover, here we mention some more contributions which regards with the generalized viscoelastic type fluids [13] - [20] .

In 2008, Zafar [21] developed a novel integral transform known as N-transform which is considered to be the generalization of famous Laplace transform as well as to Sumudu transform. Zafar applied the N-transform to a fluid problem successfully and gets some interesting results. In 2012, Belgacem [22] explain the properties and applications of this new transform and give a second name to it, the Natural transform. The properties are found to be similar to that of Laplace transform. Researchers show less attention toward Natural transform, some related studies are [23] [24] [25] .

Definition: Let $f\left(t\right)$ is defined for all $t\ge 0$ . The N-transform of $f\left(t\right)$ is the function $\overline{f}\left(c,s\right)$ defined by

${\overline{u}}_s\left(c,s\right)=N\left(u\left(t\right)\right)={\displaystyle {\int }_0^{\infty }u\left(ct\right){\text{e}}^{-st}\text{d}t},s,c\in \left(-\infty ,\infty \right)$ .

The Fox function, also referred as the Fox’s H-function, generalizes the Mellin-Barnes function. The importance of the Fox function lies in the fact that it includes nearly all special functions occurring in applied mathematics and statistics as special cases. In 1961, Fox defined the H-function as the Mellin-Barnes type path integral:

$\begin{array}{l}H\begin{array}{c}1,p\\ p,q+1\end{array}\left\{-X|\begin{array}{c}\left(1-a_1,A_1\right),\cdots ,\left(1-a_p,A_p\right)\\ \left(0,1\right)\left(1-b_{1,}{B}_1\right),\cdots ,\left(1-b_q,B_q\right)\end{array}\right\}\\ ={\displaystyle \sum _{k=1}^{\infty }\frac{\text{Γ}\left(a_1+A_{1}K\right)\cdots \text{Γ}\left(a_p+A_{p}K\right)}{\text{k}!\text{Γ}\left(b_1+B_{1}K\right)\cdots \text{Γ}\left(b_p+B_{p}K\right)}{X}^k}.\end{array}$

Researchers show less attention for the flows of Jeffrey fluids in which the fractional derivatives are appeared. We discuss three different problems related with fractional Jeffrey fluid. In the first problem we assume that the plate is jerked suddenly, in the second problem the plate is moving with uniform acceleration, and in the last problem the plate is moving with non-uniformly acceleration. In this paper we establish exact solutions for the velocity field and the associated shear stress corresponding to the unsteady flow of an incompressible generalized Jeffrey fluid between two side walls perpendicular to the plate. The obtained solutions, expressed under series form in terms of Fox H-functions [26] , are established by means of Fourier sine and N-transforms. The similar solutions for ordinary Jeffrey fluids can be obtained as limiting cases of general solutions. Finally, the influence of the fractional parameters on the motion of generalized Jeffrey fluids is underlined by graphical illustrations.

2. Governing Equations

For an incompressible and unsteady generalized Jeffrey fluid the Cauchy stress tensor is defined as [27]

$T=-pI+S,\left(1+\lambda \right)S=\mu \left(A+{\theta }^{\beta }\left(\frac{D^{\beta }}{D{t}^{\beta }}+\left(V\cdot \nabla \right)A\right)\right)$ , (1)

where S is the extra stress tensor I is the indeterminate spherical stress, μ is the dynamic viscosity, $A=L+L^T$ is the first Rivlin-Ericksen tensor, L is the velocity gradient, λ and θ are relaxation and retardation times, β is the fractional calculus parameter such that $0\le \beta \le 1$ , $D_t^{\beta }$ is the fractional differentiation operator of order β based on the Riemann-Liouville definition, defined as [8] [9]

$D_t^{\beta }\left[f\left(t\right)\right]=\frac{1}{\Gamma \left(1-p\right)}\frac{\text{d}}{\text{d}t}\underset{0}{\overset{t}{{\displaystyle \int }}}\frac{f\left(\tau \right)}{{\left(t-\tau \right)}^p}\text{d}\tau ,0<p<1$ , (2)

where $\Gamma (.)$ stands for gamma function. Model for ordinary Jeffrey fluid can be obtained by letting $\beta =1$ . For the following problem we consider the velocity field and an extra stress of the form

$V=V\left(y,z,t\right)=u\left(y,z,t\right)i,S=S\left(y,z,t\right)$ , (3)

where u is the velocity and i is the unit vector along the x-direction. The continuity equation for such flows is automatically satisfied. We take the extra stress S independent of x as the velocity field is independent of x. Also, at t = 0 the fluid being at rest is given by

$S\left(y,z,0\right)=0$ , (4)

therefore from Equations (1) and (2) it results that $S_{yy}=S_{yz}=S_{zz}=0$ and the relevant equations

$\left(1+\lambda \right){\tau }_1=\mu \left(1+{\theta }^{\beta }\frac{D^{\beta }}{D{t}^{\beta }}\right){\partial }_{y}u\left(y,z,t\right)$ , (5)

$\left(1+\lambda \right){\tau }_2=\mu \left(1+{\theta }^{\beta }\frac{D^{\beta }}{D{t}^{\beta }}\right){\partial }_{z}u\left(y,z,t\right),$ (5a)

where ${\tau }_1=S_{xy}$ and ${\tau }_2=S_{xz}$ are the tangential stresses. In the absence of body forces the balance of linear momentum becomes

${\partial }_y{\tau }_1+{\partial }_z{\tau }_2-{\partial }_{x}p=\rho {\partial }_{t}u,{\partial }_{y}p={\partial }_{z}p=0,$ (6)

here ${\partial }_{x}p$ is the pressure gradient and $\rho$ represents the density of the fluid. Eliminating the shear stresses ${\tau }_1$ and ${\tau }_2$ between Equations (5) and (6) and neglecting the pressure gradient, the governing equation reduces to the following form

$\left(1+\lambda \right)\frac{\partial }{\partial t}u\left(y,z,t\right)=v\left(1+{\theta }^{\beta }{D}_t^{\beta }\right)\left(\frac{{\partial }^2}{\partial y^2}+\frac{{\partial }^2}{\partial z^2}\right)u\left(y,z,t\right),$ (7)

where υ represents the kinematic viscosity.

3. Statement of the Problem

We take an unsteady generalized Jeffrey fluid saturating the space above a flat plate which is perpendicular to the y-axis and lies between two side walls perpendicular to the plate. At first the fluid as well as the plane wall is at rest and at time t = 0, the fluid is set into flow by translating the bottom wall in its own plane, with a time dependent velocity Vt^m. Its velocity is of the form of Equation (3) and the governing equation is given by Equation (7). The associated initial and boundary conditions are

$u\left(y,z,0\right)={\partial }_{t}u\left(y,z,0\right)=0;y>0,0\le z\le h$

$u\left(0,z,t\right)=V{t}^m;t>0,0\le z\le h$ (8)

$u\left(y,0,t\right)=u\left(y,h,t\right)=0;y,t>0.$

The distance between the two side walls is represented by h. Moreover, the natural conditions

$u\left(y,z,t\right),{\partial }_{\text{y}}u\left(y,z,t\right)\to 0\text{as}y\to \infty ,-h\le z\le h,t>0.$ . (9)

have to be also satisfied. They are consequences of the fact that the fluid will be at rest at infinity and there is no shear along y-axis.

4. Calculation of the Velocity Field for the Impulsive Motion of Plate (m = 0)

First we multiply both sides of Equation (7) by $\sin \left(\frac{n\text{π}z}{h}\right)$ , and then integrate the

obtained result from 0 to h with respect to z, we get the following differential equation

$\left(1+\lambda \right)\frac{\partial u_n\left(y,n,t\right)}{\partial t}=v\left(1+{\theta }^{\beta }{D}_t^{\beta }\right)\frac{{\partial }^2}{\partial y^2}{u}_n\left(y,n,t\right)-v{\left(\frac{n\text{π}}{h}\right)}^2\left(1+{\theta }^{\beta }{D}_t^{\beta }\right)u_n\left(y,n,t\right)$ (10)

Applying the N-transform to Equation (10), we find that the image function ${\overline{u}}_n\left(y,n,s\right)$ of $u_n\left(y,n,t\right)$ is given by

$\frac{{\partial }^2}{\partial y^2}{\overline{u}}_n\left(y,n,s\right)-\left[{\xi }^2+\frac{s\left(1+\lambda \right)}{cv\left(1+{\theta }^{\beta }\frac{s^{\beta }}{c^{\beta }}\right)}\right]{\overline{u}}_n\left(y,n,s\right)=0,$ , (11)

${\overline{u}}_n\left(0,n,s\right)=\frac{V}{s}$ ,

${\overline{u}}_n\left(0,n,s\right)\to 0\text{as}y\to \infty$ ,

where $\xi =\frac{n\pi }{h}$ . The solution of above differential equation is in the following

form

${\overline{u}}_n=\frac{cV}{s}\exp \left[-y\sqrt{{\xi }^2+\frac{s\left(1+\lambda \right)}{cv\left(1+{\theta }^{\beta }\frac{s^{\beta }}{c^{\beta }}\right)}}\right].$ (12)

We will apply the inverse N-transform technique to obtain analytic solution for the velocity field but to avoid difficult calculations of residues and contour integrals, first we express Equation (12) in series form as

$\begin{array}{l}{\overline{u}}_n\left(y,n,s\right)=V{\displaystyle \sum _{j=0}^{\infty }{\displaystyle \sum _{n=0}^{\infty }{\displaystyle \sum _{q=0}^{\infty }{\displaystyle \sum _{p=0}^{\infty }\frac{{\left(-1\right)}^{j+n+p+q}{y}^j{\xi }^{j-2n}{v}^{-n}}{j!n!q!p!\Gamma \left(n\right)\Gamma \left(-n\right)}}}}}\\ \times \frac{{\lambda }^{n-q}{\theta }^{-n-p+\beta }\Gamma \left(p+n\right)\Gamma \left(q-n\right)\Gamma \left(n-\frac{j}{2}\right)c^{-n+\beta \left(p+n\right)+1}}{\Gamma \left(\frac{j}{2}\right)s^{-n+\beta \left(p+n\right)+1}}.\end{array}$ (13)

We apply the inverse N-transform to Equation (13), to obtain

$\begin{array}{l}{u}_n\left(y,n,s\right)=V{\displaystyle \sum _{j=0}^{\infty }{\displaystyle \sum _{n=0}^{\infty }{\displaystyle \sum _{q=0}^{\infty }{\displaystyle \sum _{p=0}^{\infty }\frac{{\left(-1\right)}^{j+n+p+q}{y}^j{\xi }^{j-2n}{v}^{-n}}{j!n!q!p!\Gamma \left(n\right)\Gamma \left(-n\right)\Gamma \left(\frac{j}{2}\right)}}}}}\\ \times \frac{{\lambda }^{n-q}{\theta }^{-n-p+\beta }\Gamma \left(p+n\right)\Gamma \left(q-n\right)\Gamma \left(n-\frac{j}{2}\right)t^{-n+\beta \left(p+n\right)}}{\Gamma \left(-n+\beta \left(p+n\right)+1\right)}.\end{array}$ (14)

Taking the inverse finite Fourier sine transform to get the analytic solution of the velocity field

$\begin{array}{l}u\left(y,z,t\right)=\frac{2}{h}{\displaystyle \sum _{m=1}^{\infty }\sin \left(\frac{m\text{π}z}{h}\right)u_n}=\frac{2V}{h}{\displaystyle \sum _{m=1}^{\infty }\sin \left(\frac{m\text{π}z}{h}\right)u_n}{\displaystyle \sum _{j=0}^{\infty }{\displaystyle \sum _{n=0}^{\infty }{\displaystyle \sum _{q=0}^{\infty }{\displaystyle \sum _{p=0}^{\infty }\frac{{\left(-1\right)}^{j+n+p+q}}{j!n!q!p!}}}}}\\ \times \frac{y^j{\xi }^{j-2n}{v}^{-n}\Gamma \left(p+n\right)\Gamma \left(q-n\right)\Gamma \left(n-\frac{j}{2}\right)t^{-n+\beta \left(p+n\right)}}{\Gamma \left(n\right)\Gamma \left(-n\right)\Gamma \left(\frac{j}{2}\right){\lambda }^{q-n}{\theta }^{n+p-\beta }\Gamma \left(-n+\beta \left(p+n\right)+1\right)}.\end{array}$ (15)

To write Equation (15) in a more compact form, we use the Fox H-function,

$\begin{array}{l}u\left(y,z,t\right)=\frac{2V}{h}{\displaystyle \sum _{m=1}^{\infty }\sin \left(\frac{m\text{π}z}{h}\right)}{\displaystyle \sum _{j=0}^{\infty }{\displaystyle \sum _{n=0}^{\infty }{\displaystyle \sum _{q=0}^{\infty }\frac{{\left(-1\right)}^{j+n+p+q}{y}^j{\xi }^{j-2n}{v}^{-n}}{j!n!q!p!{\lambda }^{q-n}{\theta }^{n-\beta }{t}^{n-\beta n}}}}}\\ \times H\begin{array}{c}1,3\\ 3,5\end{array}\left\{\frac{t^{\beta }}{\theta }|\begin{array}{c}\left(1-n,1\right),\left(1-q+n,0\right),\left(1-n+\frac{j}{2},0\right).\\ \left(0,1\right),\left(1-n,0\right),\left(1+n,0\right),\left(1-j/2,0\right),\left(n-\beta n,\beta \right).\end{array}\right\}\end{array}$ (16)

To obtain (16), the following Fox H-function property is used:

$\begin{array}{l}H\begin{array}{c}1,p\\ p,q+1\end{array}\left\{-X|\begin{array}{c}\left(1-a_1,A_1\right),\cdots ,\left(1-a_p,A_p\right)\\ \left(0,1\right)\left(1-b_{1,}{B}_1\right),\cdots ,\left(1-b_q,B_q\right)\end{array}\right\}\\ ={\displaystyle \sum _{k=1}^{\infty }\frac{\Gamma \left(a_1+A_{1}K\right)\cdots \Gamma \left(a_p+A_{p}K\right)}{k!\Gamma \left(b_1+B_{1}K\right)\cdots \Gamma \left(b_p+B_{p}K\right)}{X}^k}.\end{array}$ (17)

5. Calculation of the Shear Stress for the Impulsive Motion of Plate

To get the shear stress first we apply N-transform to Equations (5) and (5a), to obtain

$\left(1+\lambda \right){\overline{\tau }}_1=\mu \left(1+{\theta }^{\beta }\frac{s^{\beta }}{c^{\beta }}\right){\partial }_y\overline{u}\left(y,z,s\right)$ , (18)

$\left(1+\lambda \right){\overline{\tau }}_2=\mu \left(1+{\theta }^{\beta }\frac{s^{\beta }}{c^{\beta }}\right){\partial }_z\overline{u}\left(y,z,s\right)$ . (19)

Taking inverse Fourier transform of Equation (12) to get $\overline{u}\left(y,z,s\right)$ and then putting it into Equation (18), we obtain

$\begin{array}{l}{\overline{\tau }}_1=\frac{2V\xi \mu \left(1+{\theta }^{\beta }\frac{s^{\beta }}{c^{\beta }}\right)}{h\left(1+\lambda \right)}{\displaystyle \sum _{n=1}^{\infty }\sin \left(\frac{n\text{π}z}{h}\right)}\\ \times \exp \left[-y\sqrt{{\xi }^2+\frac{s\left(1+\lambda \right)}{vc\left(1+{\theta }^{\beta }\frac{s^{\beta }}{c^{\beta }}\right)}}\right]\left[\sqrt{1+\frac{s\left(1+\lambda \right)}{{\xi }^{2}vc\left(1+{\theta }^{\beta }\frac{s^{\beta }}{c^{\beta }}\right)}}\right].\end{array}$ (20)

We express Equation (20) in series form in order to obtain a more suitable form of ${\tau }_1$

$\begin{array}{l}{\overline{\tau }}_1=\frac{2V\rho v}{h}{\displaystyle \sum _{n=1}^{\infty }\sin \left(\frac{n\text{π}z}{h}\right)}{\displaystyle \sum _{j=0}^{\infty }{\displaystyle \sum _{n=0}^{\infty }{\displaystyle \sum _{q=0}^{\infty }{\displaystyle \sum _{p=0}^{\infty }{\displaystyle \sum _{w=0}^{\infty }{\displaystyle \sum _{y=0}^{\infty }{\displaystyle \sum _{z=0}^{\infty }{\displaystyle \sum _{x=0}^{\infty }{\displaystyle \sum _{m=0}^{\infty }{\theta }^{-n-p+w+x+y+z+\beta }}}}}}}}}}\\ \times \frac{y^j{\left(-1\right)}^{j+n+p+q+w+y+z+x+m}{\lambda }^{n-q}{s}^{n-\beta \left(p+n-w-y\right)-m-1/2}}{{\xi }^{-j+2n+2m}{v}^{n-m}j!n!q!p!w!y!z!x!m!c^{n-\beta \left(p+n-w-y\right)-m-1/2}}\\ \times \frac{\Gamma \left(p+n\right)\Gamma \left(q-n\right)\Gamma \left(n-j/2\right)\Gamma \left(w-\frac{1}{2}\right)\Gamma \left(x+\frac{1}{2}\right)\Gamma \left(m-\frac{1}{2}\right)\Gamma \left(y-m\right)\Gamma \left(z+m\right)}{\Gamma \left(n\right)\Gamma \left(-n\right)\Gamma \left(1/2\right)\Gamma \left(j/2\right)\Gamma \left(m\right)\Gamma \left(-m\right)\Gamma \left(1/2\right)\Gamma \left(-1/2\right)}.\end{array}$ (21)

Taking the inverse N-transform of (21), we obtain

$\begin{array}{l}{\tau }_1=\frac{2V\rho v}{h}{\displaystyle \sum _{n=1}^{n=1}\sin \left(\frac{n\text{π}z}{h}\right)}{\displaystyle \sum _{j=0}^{\infty }{\displaystyle \sum _{n=0}^{\infty }{\displaystyle \sum _{q=0}^{\infty }{\displaystyle \sum _{p=0}^{\infty }{\displaystyle \sum _{w=0}^{\infty }{\displaystyle \sum _{y=0}^{\infty }{\displaystyle \sum _{z=0}^{\infty }{\displaystyle \sum _{x=0}^{\infty }{\displaystyle \sum _{m=0}^{\infty }{\theta }^{-n-p+w+x+y+z+\beta }}}}}}}}}}\\ \times \frac{y^j{\left(-1\right)}^{j+n+p+q+w+y+z+x+m}{\lambda }^{n-q}{t}^{-n+\beta \left(p+n-w-y\right)+m+1/2}}{{\xi }^{-j+2n+2m}{v}^{n-m}j!n!q!p!w!y!z!x!m!}\\ \times \frac{\Gamma \left(p+n\right)\Gamma \left(q-n\right)\Gamma \left(n-j/2\right)\Gamma \left(w-\frac{1}{2}\right)\Gamma \left(x+\frac{1}{2}\right)\Gamma \left(m-\frac{1}{2}\right)\Gamma \left(y-m\right)\Gamma \left(z+m\right)}{\Gamma \left(j/2\right)\Gamma \left(n\right)\Gamma \left(n\right)\Gamma \left(-n\right)\Gamma \left(1/2\right)\Gamma \left(m\right)\Gamma \left(-m\right)\Gamma \left(1/2\right)\Gamma \left(-1/2\right)\Gamma \left(-n+\beta n+1/2\right)}\end{array}$ (22)

Finally, using the Fox H-function we obtain the stress field as

$\begin{array}{l}{\tau }_1=\frac{2Vv}{h}{\displaystyle \sum _{n=1}^{n=1}\sin \left(\frac{n\text{π}z}{h}\right)}{\displaystyle \sum _{j=0}^{\infty }{\displaystyle \sum _{n=0}^{\infty }{\displaystyle \sum _{q=0}^{\infty }{\displaystyle \sum _{p=0}^{\infty }{\displaystyle \sum _{w=0}^{\infty }{\displaystyle \sum _{y=0}^{\infty }{\displaystyle \sum _{z=0}^{\infty }{\displaystyle \sum _{x=0}^{\infty }{\xi }^{j-2n}}}}}}}}}\\ \times \frac{y^j{\left(-1\right)}^{j+n+p+q+w+y+z+x}{\lambda }^{n-q}{t}^{-n+\beta \left(p+n-w-y\right)+1/2}}{{\theta }^{n+p-w-x-y-z-\beta }{v}^{n}j!n!q!p!w!y!z!x!}\\ \times H\begin{array}{c}1,8\\ 8,10\end{array}\left\{\frac{-{\xi }^{2}t}{v}|\begin{array}{c}\left(1-p+n,0\right),\cdots ,\left(1-z,1\right)\\ \left(1-j/2,0\right),\cdots ,\left(1+n-\beta n,\beta \right)\end{array}\right\}\end{array}$ (23)

In the similar fashion we can find ${\tau }_2\left(y,z,t\right)$ from Equations (16) and (19).

6. Velocity Field and Shear Stress of the Flow Due to Impulsive Accelerating Plate (m = 1)

Following the procedure of the previous section, the expression for the velocity field is given by

$\begin{array}{l}u\left(y,z,t\right)=\frac{2V}{h}{\displaystyle \sum _{m=1}^{\infty }\sin \left(\frac{m\text{π}z}{h}\right)}{\displaystyle \sum _{j=0}^{\infty }{\displaystyle \sum _{n=0}^{\infty }{\displaystyle \sum _{q=0}^{\infty }\frac{{\left(-1\right)}^{j+n+p+q}{y}^j{\xi }^{j-2n}{v}^{-n}}{j!n!q!p!{\lambda }^{q-n}{\theta }^{n-\beta }{t}^{n-\beta n-1}}}}}\\ \times H\begin{array}{c}1,3\\ 3,5\end{array}\left\{\frac{t^{\beta }}{\theta }|\begin{array}{c}\left(1-n,1\right),\left(1-q+n,0\right),\left(1-n+j/2,0\right).\\ \left(0,1\right),\left(1-n,0\right),\left(1+n,0\right),\left(1-j/2,0\right),\left(1+n-\beta n,\beta \right).\end{array}\right\}\end{array}$ (24)

7. Velocity Field and Shear Stress of the Flow Due to Impulsive Accelerating Plate (m = 2)

Adopting the methodology of the previous section, the resultant expression for the velocity field is given by

$\begin{array}{l}u\left(y,z,t\right)=\frac{2V}{h}{\displaystyle \sum _{m=1}^{\infty }\sin \left(\frac{m\text{π}z}{h}\right)}{\displaystyle \sum _{j=0}^{\infty }{\displaystyle \sum _{n=0}^{\infty }{\displaystyle \sum _{q=0}^{\infty }\frac{{\left(-1\right)}^{j+n+p+q}{y}^j{\xi }^{j-2n}{v}^{-n}}{j!n!q!p!{\lambda }^{q-n}{\theta }^{n-\beta }{t}^{n-\beta n-2}}}}}\\ \times H\begin{array}{c}1,3\\ 3,5\end{array}\left\{\frac{t^{\beta }}{\theta }|\begin{array}{c}\left(1-n,1\right),\left(1-q+n,0\right),\left(1-n+j/2,0\right).\\ \left(0,1\right),\left(1-n,0\right),\left(1+n,0\right),\left(1-j/2,0\right),\left(2+n-\beta n,\beta \right).\end{array}\right\}\end{array}$ (25)

8. Special Case

By letting $\beta =1$ in Equations (16), we get the velocity profile for an ordinary Jeffrey fluid induced by the impulsive motion of the plate

$\begin{array}{l}u\left(y,z,t\right)=\frac{2V}{h}{\displaystyle \sum _{m=1}^{\infty }\sin \left(\frac{m\text{π}z}{h}\right)}{\displaystyle \sum _{j=0}^{\infty }{\displaystyle \sum _{n=0}^{\infty }{\displaystyle \sum _{q=0}^{\infty }\frac{{\left(-1\right)}^{j+n+p+q}{y}^j{\xi }^{j-2n}{v}^{-n}}{j!n!q!p!{\lambda }^{q-n}{\theta }^{n-1}}}}}\\ \times H\begin{array}{c}1,3\\ 3,5\end{array}\left\{\frac{t}{\theta }|\begin{array}{c}\left(1-n,1\right),\left(1-q+n,0\right),\left(1-n+j/2,0\right).\\ \left(0,1\right),\left(1-n,0\right),\left(1+n,0\right),\left(1-j/2,0\right),\left(n-n,1\right).\end{array}\right\}\end{array}$ (26)

Similarly, we can get velocity field for an ordinary Jeffrey fluid due to impulsive accelerating plate and non-uniformly accelerating plate.

9. Numerical Results and Discussion

We have presented unsteady flows of a generalized Jeffrey fluid induced by impulsive motion of the plate between two side walls perpendicular to the plate. Exact analytical solutions are established for such flow problem using Fourier sine and N-transforms technique. The obtained solutions are expressed in series form using Fox H-functions. Several graphs are presented here for the analysis of some important physical aspects of the obtained solutions. The corresponding solutions for ordinary Jeffrey fluid is also obtained as limiting case of our general solutions. The numerical results show the profiles of velocity and the adequate shear stress for the flow. We analyze these results by changing different parameters of interest.

The effects of fractional parameters β of the model are important for us to be discussed. In Figure 1 we depict the profiles of velocity and shear stress for three different values of β. It is observed from these figures that the flow velocity as well as the shear stress increases with increasing β, which corresponds to the shear thinning phenomenon. Figure 2 are sketched to show the velocity and the shear stress profiles at different values of λ. It is noticeable that velocity as well as the shear stress decreases by increasing λ. In order to study the effects of material parameter θ, we have plotted Figure 3, where it appears that the velocity is also a strong function of the material parameter θ of Jeffrey fluid. It can be observed that the increase of material parameter θ acts as an increase of the magnitude of velocity components near the plate, and this again corresponds to the shear-thinning behavior of the examined non-Newtonian fluid. Figure 4 presents, the velocity field and the shear stress profiles at different values of y. It

is noticeable that velocity and shear stress decreases by increasing y. Also, by increasing y the velocity becomes steady, which shows that the boundary condition (9) is satisfied.

10. Conclusion

In this paper, a new transform is used to obtain some exact solutions regarding Jeffrey fluid model. The N-transform is actually a generalization of Laplace transform. Fractional differential equation is involved in the governing equation, which is solved for the velocity with the help of finite Fourier transform. The flow is set into motion with the help of flat plat which is lying between two perpendicular plates. The series solution of velocity field and the associated shear stress in terms of Fox H-functions, satisfying all imposed initial and boundary

conditions have been obtained. The similar solutions for ordinary Jeffrey fluid, performing the same motion, appear as limiting case of the solutions are obtained here. Also, the obtained results are analyzed graphically through various pertinent parameters. Furthermore, the obtained solutions satisfy the governing equations and all imposed initial and boundary conditions.

Cite this paper

Khan, A., Zaman, G., Ahmad, S. and Chohan, M.I. (2017) Some Exact Solutions of Generalized Jeffrey Fluid Using N-Transform. American Journal of Computational Mathematics, 7, 402-412. https://doi.org/10.4236/ajcm.2017.74029

References