# Analytical Solution of MHD Stagnation-Point Flow and Heat Transfer of Casson Fluid over a Stretching Sheet with Partial Slip

Authors: Samir Kumar Nandy
Journal: ISRN Thermodynamics
 (2013)

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## Abstract

This paper investigates the hydromagnetic boundary layer flow and heat transfer of a non-Newtonian Casson fluid in the neighborhood of a stagnation point over a stretching surface in the presence of velocity and thermal slips at the boundary. The governing partial differential equations are transformed into nonlinear ordinary differential equations using similarity transformations. The analytic solutions are developed by a homotopy analysis method (HAM). The results pertaining to the present study indicate that the flow and temperature fields are significantly influenced by Casson parameter (β), the magnetic parameter M, the velocity slip parameter δ, and the thermal slip parameter γ. An increase in the velocity slip parameter δ causes decrease in the flow velocity, while an increase in the value of the thermal slip parameter γ causes increase in the temperature of the fluid. It is also observed that the velocity at a point decreases with increase in β.


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## Body

## 1. Introduction

The problems of flow and heat transfer in the boundary layer adjacent to a continuous moving surface have received great attention during the last decades owing to the abundance of practical applications in chemical and manufacturing processes, such as polymer extrusion, continuous casting of metals, glass fibre production, hot rolling of paper, and wire drawing. Sakiadis [1] was the first, among others, to investigate the flow behavior on continuous solid surface. Thereafter, numerous investigations were made on the flow and heat transfer over a stretching surface in different directions [2–8].All the previous researchers restricted their analyses to flow and heat transfer for the Newtonian fluid. In recent years, it has been observed that a number of industrial fluids such as molten plastics, polymeric liquids, blood, food stuff, and slurries exhibit non-Newtonian fluid behavior. Different types of non-Newtonian fluids are viscoelastic fluid, couple stress fluid, micropolar fluid, power-law fluid, Casson fluid, and many others. Rajagopal et al. [9] and Siddappa and Abel [10] studied the flow of a viscoelastic fluid over a linear stretching sheet. Troy et al. [11], Lawrence and Rao [12], and McLeod and Rajagopal [13] discussed the problem of uniqueness/nonuniqueness of the flow of a non-Newtonian viscoelastic fluid over a stretching sheet. Rajagopal et al. [9] analyzed the solutions for the flow of viscoelastic fluid over a stretching sheet. This study was further generalized to investigate the flow of short memory fluid of type Walter's liquid B by several authors, such as Andersson [14], Rollins and Vajravelu [15], and Abel and Veena [16].Although different models are proposed to explain the behavior of non-Newtonian fluids, the most important non-Newtonian fluid possessing a yield value is the Casson fluid. This fluid has significant applications in polymer processing industries and biomechanics. We can define a casson fluid as a shear thinning fluid which is assumed to have an infinite viscosity at zero rate of shear. Casson's constitutive equations are found to describe accurately the flow curves of suspensions of pigments in lithographic varnishes used for preparation of printing inks and silicon suspensions [17]. Various experiments performed on blood with varying haematocrits, anticoagulants, temperatures, and so forth strongly suggest the behavior of blood as a casson fluid [18–20]. In particular, casson fluid model describes the flow characteristics of blood more accurately at low shear rates and when it flows through small vessels [21].Fluid flow in microelectromechanical systems (MEMS) has become an interesting topic because in microscale dimensions, the fluid flow behavior deviates significantly from the traditional no-slip flow. Under the microscale dimensions, the fluid motion still obeys the Navier-Stokes equations but under slip velocity boundary conditions. For large scale problems with low density, the fluid can be modeled as a rarefied gas, and rarefied gas flows with slip boundary conditions are often countered in the microscale devices. The nonadherence of the fluid to a solid boundary, known as velocity slip, is a phenomenon observed in certain circumstances. Partial slips occur for fluids with particulate such as emulsions, suspensions, foams, and polymer solutions. Fluids exhibiting slip are important in technological applications such as in the polishing of artificial heart valves and internal cavities. With a slip at the wall boundary, the flow behavior and the shear stress in the fluid are quite different from those in the no-slip flows. The slip flows in different flow configurations were studied in recent years (see [22–27]). The MHD flow under slip conditions over a permeable shrinking surface was solved analytically by Fang et al. [28], and they reported that the velocity slip at the shrinking surface greatly affects the velocity distribution and drag forces on the wall. Bhattacharyya et al. [29] studied the effects of partial slip on the boundary layer stagnation-point flow and heat transfer towards a shrinking surface. The slip effect on MHD boundary layer flow over a flat plate was also considered by Bhattacharyya et al. [30]. Ariel et al. [31] considered the flow of a viscoelastic fluid over a stretching sheet with partial slip, and Ariel [32] also studied the slip effect on stagnation-point flow of an elasticoviscous fluid over a wall. Fang et al. [33] obtained the exact analytic solution of MHD flow under slip condition over a permeable stretching sheet.However, in the literature, articles are not available on the MHD boundary layer stagnation-point flow of a casson fluid over a stretching sheet. The present paper aims to study the slip effect on MHD boundary layer flow and heat transfer of a casson fluid over a stretching sheet using the homotopy analysis method (HAM) which is successively applied to various interesting problems [34–41]. The self-similar equations are solved analytically by HAM for a range of values of the physical parameters. The results obtained are then compared with those from the available literature for some particular values of the physical parameters, and it is found that they are in a good agreement. The results pertaining to the present study indicate that the flow and the temperature fields are greatly influenced by the velocity and thermal slip parameters.


## 2. Flow Analysis

Consider the steady magnetohydrodynamic (MHD) flow of a non-Newtonian Casson fluid near the stagnation point over a stretching surface coinciding with the planey=0, the flow being confined to y>0. Two equal and opposite forces are applied along the x-axis so that the surface is stretched keeping the origin fixed. A uniform magnetic field of strength B0 is applied in a direction normal to the surface. It is assumed that the velocity distribution far from the surface is given by u→U(x)=ax, where a(>0) is a constant. The stretching surface has a uniform temperature Tw and the temperature far away from the surface is T∞. The flow configuration is shown in Figure 1.Figure 1
A physical model and the coordinate system.The rheological equation of state for an isotropic and incompressible flow of a Casson fluid can be written as, see Nakamura and Sawada [42],
(1)τij=2(kc+τ02π)eij,π>πc,τij=2(kc+τ02πc)eij,π<πc,
where
(2)eij=12(∂ui∂xj+∂uj∂xi)
is the rate-of-strain tensor, kc is the Casson's coefficient of viscosity, π is the product of the component of deformation rate with itself, πc is the critical value of the product of the component of the rate-of-strain tensor with itself, τ0 is the yield stress of the fluid, and ui are the velocity components.The MHD equations for this problem in the boundary layer near the stretching surface are(3)∂u∂x+∂v∂y=0,(4)u∂u∂x+v∂u∂y=UdUdx+ν(1+1β)∂2u∂y2+σB02ρ(U-u),(5)u∂T∂x+v∂T∂y=κ∂2T∂y2+νcp(1+1β)(∂u∂y)2+σB02ρcp(U-u)2,
where u and v are the velocity components along the x and y directions, respectively, ρ is the density of the fluid, σ is the electrical conductivity, B0 is the uniform magnetic field along y-axis, κ is the thermal diffusivity, cp is the specific heat at constant pressure, ν is the kinematic viscosity, and β(=kc2πc/τ0) is the Casson parameter. In writing (4), we have neglected the induced magnetic field since the magnetic Reynolds number RM for the flow is assumed to be very small. This assumption is justified for flow of electrically conducting fluids such as liquid metals, for example, mercury, liquid sodium, and so forth (Shercliff [43]).The slip boundary conditions for the problem are(6)u=cx+L∂u∂y,v=0,T=Tw+S∂T∂yaty=0,u⟶U(x)=ax,T⟶T∞asy⟶∞,
where L is the velocity slip factor, S is the thermal slip factor, and a(>0), c(>0) are constants. For L=0 and S=0, no-slip condition can be recovered.The continuity equation can be satisfied by introducing a stream functionψ such that
(7)u=∂ψ∂y,v=-∂ψ∂x.
The momentum and energy equations can be transformed into the corresponding nonlinear ordinary differential equations by the following transformations:
(8)ψ=xcνF(η),θ(η)=T-T∞Tw-T∞,η=ycν,
where η is the independent similarity variable and where Tw-T∞=bx2, b is a positive constant. Using these relations, we get the transformed nonlinear ordinary differential equations from (4) and (5) as
(9)(1+1β)F′′′+FF′′-F′2+α2+M(α-F′)=0,(10)1Prθ′′+Fθ′-2F′θ+(1+1β)EcF′′+MEc(α-F′)2=0,
where α(=a/c) is the dimensionless velocity ratio parameter, M(=σB02/ρc) is the magnetic parameter, Pr=(ν/κ) is the Prandtl number, Ec(=c2/bcp) is the Eckert number, and a prime denotes differentiation with respect to the similarity variable η. The transformed boundary conditions for F(η) and θ(η) are
(11)F(0)=0,F′(0)=1+δF′′(0),θ(0)=1+γθ′(0),F′(∞)=α,θ(∞)=0,
where δ=(c/ν)1/2L is the dimensionless velocity slip parameters γ=(c/ν)1/2S is the dimensionless thermal slip parameter. It is to be noted that when the non-Newtonian (Casson) parameter β→∞, the Casson flow problem reduces to viscous flow problem.The physical quantities of interest are the skin friction coefficientCF and the local Nusselt number Nux, which are defined as
(12)CF=τwρuw2(x),Nux=xqwk(Tw-T∞),
where τw is the shear stress along the stretching surface and qw is the heat flux from the stretching surface, which are given by
(13)τw=(kc+τ02πc)(∂u∂y)y=0,qw=-k(∂T∂y)y=0.
Hence using (8) we get
(14)Rex1/2CF=(1+1β)F′′(0),NuxRex1/2=-θ′(0),
where Rex=uw(x)x/ν is the local Reynolds number.


## 3. Analytical Solutions forF(η) and θ(η)

For the explicit analytical solution of (9)–(11) by Homotopy Analysis Method (HAM), the velocity F(η) and the temperature θ(η) distributions can be expressed by the set of base functions
(15){ηmexp(-nη):m≥0,n≥0areintegers}
in the form:
(16)F(η)=a0,00+∑n=0∞‍∑m=0∞‍ak,nmηmexp(-nη),θ(η)=∑n=0∞‍∑m=0∞‍bk,nmηmexp(-nη),
where ak,nm and bk,nm are coefficients. Then from (16) and the boundary conditions (11), it is straightforward to choose
(17)F0(η)=αη+(1-α1+δ)[1-exp(-η)],θ0(η)=exp(-η)1+γ,
as our initial approximations for F(η) and θ(η), respectively. We choose the auxiliary linear operators as
(18)LF(F)=∂3F∂η3+∂2F∂η2,Lθ(θ)=∂2θ∂η2-θ,
with the properties
(19)LF[C1+C2η+C3exp(-η)]=0,Lθ[C4exp(η)+C5exp(-η)]=0,
where Ci(i=1-5) are constants. Let q∈[0,1] be an embedding parameter and hF, hθ denote the nonzero auxiliary linear operators, then the zeroth order deformation equations are
(20)(1-q)LF[F^(η;q)-F0(η)]=qhFNF[F^(η;q)],(1-q)Lθ[θ^(η;q)-θ0(η)]=qhθNθ[F^(η;q),θ^(η;q)],
subject to the boundary conditions
(21)F^(η;q)|η=0=0,∂F^(η;q)∂η|η=0=1+δ∂2F^(η;q)∂η2|η=0,∂F^(η;q)∂η|η=+∞=ac,(22)θ^(η;q)|η=0=1+γ∂θ^(η;q)∂η|η=0,θ^(η;q)|η=∞=0,
where the nonlinear operators NF and Nθ are defined as
(23)NF[F^(η;q)]=(1+1β)∂3F^(η;q)∂η3+F^(η;q)∂2F^(η;q)∂η2-(∂F^(η;q)∂η)2+α2+M[α-∂F^(η;q)∂η],Nθ[F^(η;q),θ^(η;q)]=1Pr∂2θ^(η;q)∂η2+F^(η;q)∂θ^(η;q)∂η-2∂F^(η;q)∂ηθ^(η;q)+(1+1β)Ec∂2F^(η;q)∂η2+MEc(α-∂F^(η;q)∂η)2.
When q=0, we have from (20) that
(24)F^(η,0)=F0(η),θ^(η,0)=θ0(η).
When q=1, the zeroth order deformation equations (20)–(22) are equivalent to the original equations (9)–(11) so that we have
(25)F^(η,1)=F(η),θ^(η,1)=θ(η).
So as the embedding parameter q increases from 0 to 1, F^(η,q) and θ^(η,q) vary from their initial approximations F0(η) and θ0(η) to their exact solutions F(η) and θ(η), respectively. Expanding F^(η,q) and θ^(η,q) in Taylor series with respect to the embedding parameter q, we can write
(26)F^(η,q)=F0(η)+∑m=1∞‍Fm(η)qm,(27)θ^(η,q)=θ0(η)+∑m=1∞‍θm(η)qm,
where
(28)Fm(η)=1m!∂mF^(η;q)∂qm|q=0,θm(η)=1m!∂mθ^(η;q)∂qm|q=0.
Note that the zero order deformation equations (20) contain nonzero auxiliary parameters hF and hθ, respectively. Thus F^(η,q) and θ^(η,q) are dependent upon these parameters. Assume that hF and hθ are so chosen that the series (26) and (27) are convergent at q=1. Hence we have from (25)–(27),
(29)F(η)=F0(η)+∑m=1∞‍Fm(η),θ(η)=θ0(η)+∑m=1∞‍θm(η).
Differentiating the zeroth-order deformation equations (20)–(22) m times with respect to q and then dividing by m! and finally setting q=0, we have the mth order deformation equations as
(30)LF[Fm(η)-χmFm-1(η)]=hFRmF(η),(31)Lθ[θm(η)-χmθm-1(η)]=hθRmθ(η),(32)Fm(0)=Fm′(0)-δFm′′(0)=Fm′(∞)=0,θm(0)-γθm′(0)=θm(∞)=0,
where
(33)RmF(η)=(1+1β)F′′′+∑k=0m-1‍[Fm-1-kFk′′-Fm-1-k′Fk′]-MFm-1′+(Mα+α2)(1-χm),Rmθ(η)=1Prθm-1′′+∑k=0m-1‍Fm-1-kθk′-2∑k=0m-1‍Fm-1-k′θk+(1+1β)Ec∑k=0m-1‍Fm-1-k′′Fk′′+(1-χm)MEcα2-2MEcαFm-1′+MEc∑k=0m-1‍Fm-1-k′Fk′,χm={0m≤11m≥2.
The general solutions of (30)–(32) are
(34)Fm(η)=Fm*(η)+C1+C2η+C3exp(-η),θm(η)=θm*(η)+C4exp(η)+C5exp(-η),
where Fm*(η) and θm*(η) denote the special solutions of (30) and (31) and the integral constants Ci(i=1,2,3,4,5) are determined by the following boundary conditions:
(35)C2=C4=0,C3=11+δ[∂Fm*(η)∂η|η=0-δ∂2Fm*(η)∂η2|η=0],C1=-C3-Fm*(0),C5=11+γ[γ∂θm*(η)∂η|η=0-θm*(0)].
The linear mth order deformation equations (30) and (31) can be solved one after the other by using the symbolic computation software MATHEMATICA.


## 4. Convergence of the HAM Solution

Equation (29) gives the analytical solution of the problem in series form. As pointed out by Liao [35], the convergence region and rate of convergence of the solution series given by HAM depend upon auxiliary parameters hF and hθ. Hence these auxiliary parameters provide us with a convenient way to adjust and control the convergence region and rate of the solution series. To select appropriate values of these parameters, we display the so called hF and hθ curves at 20th order approximations. Figure 2 reveals that there exists horizontal line segment for (hF,F′′(0)) curves in -0.8≤hF≤-0.3 and for (hθ,θ′′(0)) curve in -0.85≤hθ≤0.25. The obtained series solutions given by (29) converge in the whole region of η when hF=hθ=-0.3. Here we have employed the homotopy-Pade approximation (see Mahapatra et al. [40]) instead of traditional-Pade approximation for the rapid convergence of the series solutions. Table 1 is made to show the convergence of the solutions for F′′(0) and -θ′(0) using homotopy-Pade approximation.Table 1
Convergence solution for different order of approximations whenβ=1.0, α=0.5, M=1.0, δ=0.5, Pr=0.7, γ=0.3, and Ec=0.1.
Order of approximations
-
F
′
′
(
0
)
-
θ
′
(
0
)
1
0.302781
0.405632
5
0.342341
0.437431
10
0.362178
0.457285
20
0.362489
0.457285
30
0.362489
0.457285
40
0.362489
0.457285Figure 2
h curve for F′′(0) and θ′(0).


## 5. Results and Discussion

Equations (9) and (10) subject to the boundary conditions (11) are solved analytically for some values of the governing parameters β, α, M, Pr, Ec, δ, and γ. In order to verify the accuracy of the present method, we have compared our results with those of Mahapatra and Gupta [4] and Ishak et al. [6] for the skin friction coefficient F′′(0) for different values of α (in the case of β→∞,  M=0 and δ=0) in Table 2. The comparison shows good agreement for each value of α. Therefore, the present results obtained are accurate enough.Table 2
Comparison of the values ofF′′(0) (with β→∞) for different values of α(=a/c) with M=0 and δ=0.
α
Present study
Mahapatra and Gupta [4]
Ishak et al. [6]
0
.
01
-
0.998024
—
-
0.9980
0.10
-
0.969386
-
0.9694
-
0.9694
0.20
-
0.918107
-
0.9181
-
0.9181
0.50
-
0.667264
-
0.6673
-
0.6673
1.0
0
0
0
2.0
2.017507
2.0175
2.0175This section describes the influence of some important physical parameters on the velocity and thermal profiles. For this purpose, Figures3–11 are displayed. Attention is focussed on variations of the velocity slip parameter δ, the magnetic parameter M, the thermal slip parameter γ, the casson parameter β, the velocity ratio parameter α, and the Prandtl number Pr on the velocity and the temperature distributions.Figure 3
Influence of the velocity slip parameterδ on F′.Figure 4
Influence of the magnetic parameterM on F′.Figure 5
Influence of the Casson parameterβ on F′.Figure 6
Influence of the velocity ratio parameterα on F′.Figure 7
Influence of the thermal slip parameterγ on θ(η).Figure 8
Influence of the magnetic parameterM on θ(η).Figure 9
Influence of the velocity ratio parameterα on θ(η).Figure 10
Influence of the Prandtl numberPr on θ(η).Figure 11
Influence of the Eckert numberEc on θ(η).Figure3 shows the influence of δ on the velocity component F′. It is observed that F′ is a decreasing function of the slip parameter δ. Physically this is explained as follows: when slip occurs (for nonzero value of δ), the fluid velocity near the sheet is no longer equal to the sheet stretching velocity; that is, a velocity slip exists. With the increase in δ, such a slip velocity increases. Furthermore, increasing the value of δ will decrease the flow velocity because under the slip condition, the pulling of the stretching sheet can be only partly transmitted to the fluid. The boundary layer thickness also decreases as the slip parameter δ increases. The effect of the magnetic field parameter M on velocity F′ is depicted in Figure 4. From this figure, it is observed that the transverse magnetic field contributes to the reduction in the velocity profile and boundary later thickness. This is evident from the fact that applied transverse magnetic field produces a body force, to be precise, the Lorentz force, which opposes the motion. The resistance offered to the flow is responsible in decreasing the fluid velocity. The influence of the Casson parameter β on the velocity profile is displayed in Figure 5. The figure reveals that as β increases, the velocity and the boundary layer thickness decrease. Hence, it is quite obvious that the magnitude of the velocity is greater in casson fluid when compared with the viscous fluid. The effect of the velocity ratio parameter α on the velocity field F′ is shown in Figure 6. The figure indicates that fluid velocity increases with the increase of α.To see the variations ofγ, M, α, Pr (Prandtl number), and Ec(Eckert number) on the temperature profile θ, Figures 7–11 are plotted. The effect of the thermal slip parameter γ on temperature distribution is displayed in Figure 7. As the thermal slip increases, less heat is transferred from the sheet to the fluid and consequently the temperature decreases. Figure 8 depicts the effect of M on temperature θ. It is observed that temperature and the thermal boundary layer thickness increase with increasing M. Figure 9 exhibits the temperature profile θ for different values of the velocity ratio parameter α. The figure shows that the temperature and the thermal boundary layer thickness decrease with an increase in α. Hence, stronger free stream velocity causes a reduction in the temperature and the thermal boundary layer thickness.Figure10 demonstrates the effect of the Prandtl number Pr on the temperature profile θ. The temperature and the thermal boundary layer thickness decrease with the increase of Pr. Physically this is explained as follows. An increase in the Prandtl number means an increase of fluid viscosity, which causes a decrease in the temperature distribution. An enhancement in the Eckert number Ec results in an increase in temperature θ, and this observation can easily be visualized in Figure 11.Tables3 and 4 show the variation of the reduced skin friction coefficient F′′(0) and the coefficient of the reduced Nusselt number -θ′(0) for different values of the physical parameters β, M, α, and Pr considering other parameters fixed. From Table 3, it is observed that |F′′(0)| is an increasing function of the dimensionless parameters β and M. Also |F′′(0)| decreases with the increase of α as long as α<1 and increases with the increase of α for α>1. Table 4 reveals that -θ′(0) is a decreasing function of β and M while an increasing function of Pr.Table 3
Values ofF′′(0) for different values of β, M, and α with δ=0.5.
β
M
α
→
0.01
0.2
0.5
1.5
2.0
0.5
0.1
-
0.426217
-
0.386951
-
0.275757
0.353516
0.762695
0.5
-
0.486374
-
0.427637
-
0.296141
0.365707
0.782862
1.0
-
0.546294
-
0.469744
-
0.317999
0.379546
0.806099
1.0
0.1
-
0.491127
-
0.445542
-
0.316722
0.401925
0.863115
0.5
-
0.558715
-
0.490648
-
0.338915
0.414637
0.883828
1.0
-
0.625100
-
0.536776
-
0.362489
0.428997
0.907599Table 4
Values of-θ′(0) for different values of β, M, and Pr with δ=0.5, γ=0.3, α=0.2, and Ec=0.1.
β
M
Pr
→
0.1
0.5
0.71
2.0
5.0
0.5
0.1
0.147355
0.355671
0.423755
0.675504
0.956279
0.5
0.141579
0.340118
0.404804
0.646344
0.912599
1.0
0.136239
0.324898
0.386483
0.616944
0.868322
1.0
0.1
0.140813
0.341966
0.409257
0.662231
0.948732
0.5
0.135781
0.327236
0.391145
0.634582
0.908910
1.0
0.131151
0.312713
0.374024
0.607155
0.869149


## 6. Conclusion

The present work considers the hydromagnetic steady flow and heat transfer of a non-Newtonian casson fluid in the neighborhood of a stagnation point over a stretching surface with partial slip at the boundary. The governing equations are formulated and transformed into a set of ordinary differential equations by similarity transformation. The resulting equations are solved analytically using homotopy analysis method. The main points of this study are as follows.(i)
The velocityF′ decreases with increasing values of δ, M, and β.(ii)
The temperatureθ decreases with increasing values of γ, α, and Pr, and increases with increasing values of M and Ec.(iii)
The magnitude of velocity is greater in case of Casson fluid when compared with the viscous fluid.(iv)
Increase of the velocity slip parameterδ causes decrease in the flow velocity, and the same qualitative result holds for the thermal slip parameter γ on the temperature.(v)
The present results in limiting cases (β→∞,M=0,δ=0) are found in excellent agreement with those of Mahapatra and Gupta [4] and Ishak et al. [6].



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