Mathematical Problems in Engineering

Mathematical Problems in Engineering / 2011 / Article

Research Article | Open Access

Volume 2011 |Article ID 132457 | 17 pages | https://doi.org/10.1155/2011/132457

Steady Thermal Analysis of Two-Dimensional Cylindrical Pin Fin with a Nonconstant Base Temperature

Academic Editor: Jerzy Warminski
Received31 Mar 2011
Revised13 Jun 2011
Accepted28 Jun 2011
Published04 Sep 2011

Abstract

Steady heat transfer through a pin fin is studied. Thermal conductivity, heat transfer coefficient, and the source or sink term are assumed to be temperature dependent. In the model considered, the source or sink term is given as an arbitrary function. We employ symmetry techniques to determine forms of the source or sink term for which the extra Lie point symmetries are admitted. Method of separation of variables is used to construct exact solutions when the governing equation is linear. Symmetry reductions result in reduced ordinary differential equations when the problem is nonlinear and some invariant solution for the linear case. Furthermore, we analyze the heat flux, fin efficiency, and the entropy generation.

1. Introduction

Fins play an important role in increasing the efficiency of heating systems which is achieved by increased (extended) surface area. In particular, fins are used in power generators, air conditioning, semiconductors, refrigeration, cooling of computer processor, exothermic reactors, and many other devices in which heat is generated and must be transported. Theory, solutions and applications of problems on extended surfaces may be found in texts such as [1].

One-dimensional steady state numerical analysis have been considered, for example, by [2–5], and exact solutions were constructed via symmetry techniques in [6]. The transient one-dimensional fin problem has attracted sizeable interest from the Lie symmetry analysts (see, e.g., [7–11]). Two-dimensional transient analysis have been carried out for fins without heat source or sink in [12]. Solutions for two-dimensional fin models exist for the constant thermal conductivity (see e.g., [13–16]). Recently, heat transfer and entropy generation in two-dimensional orthotropic pin fin has been studied in [17]. In [18], the authors combined the Laplace transformation and the finite difference methods to determine solutions for the two-dimensional pin fins with nonconstant base heat flux. A search for exact and numerical solutions for heat transfer in extended surfaces continues to be of scientific interest. perhaps the interest is instilled by frequent encounters in many engineering applications. To cite a few, some other contributions of heat flow particularly in pin fins may be found, for example, in [19, 20].

In this paper, we consider the steady heat flow through a two-dimensional pin fin with a temperature-dependent internal heat generating or extracting function and thermal conductivity. Furthermore, heat is transferred at the boundary through the temperature-dependent heat transfer coefficient. Symmetry analysis is employed to determine all possible forms of the source or sink term for which the problem is at least reducible to ordinary differential equations. The paper is arranged as follows: in Section 2, we provide mathematical formulation of the problem. Section 3 deals with the symmetry analysis, and exact solutions are constructed in Section 4. The fin efficiency and heat flux are given in Section 5. Entropy analysis is carried out in Section 6. Lastly, we provide the discussions in Section 7 and concluding remarks in Section 8.

2. Mathematical Formulation

We consider a two-dimensional pin fin with length 𝐿 and radius 𝑅. The fin is attached to a base surface of temperature (ğ‘‡ğ‘âˆ’ğ‘‡âˆž)𝑔(𝑅) and extended into the fluid of temperature ğ‘‡âˆž. The tip of the fin is insulated (i.e., heat transfer at the tip is negligibly small). The fin is measured from the tip to the base. A schematic representation of a pin fin is given in Figure 1. We assume that the heat transfer coefficient along the fin is nonuniform and temperature dependent and that the fin has internal heat source or sink. Furthermore, the temperature-dependent thermal conductivity is assumed to be the same in both radial and axial directions. The base temperature is assumed to be nonconstant (see, e.g., [19, 20]). The energy balance equation is written as1𝑅𝜕𝜕𝑅𝑅𝐾(𝑇)𝜕𝑇+𝜕𝜕𝑅𝜕𝑋𝐾(𝑇)𝜕𝑇𝜕𝑋=𝑆(𝑇).(2.1) The boundary conditions are𝜕𝑇𝜕𝑋=0,𝑋=0,0â‰¤ğ‘…â‰¤ğ‘…ğ‘Ž,ğ‘‡âˆ’ğ‘‡âˆž=î€·ğ‘‡ğ‘âˆ’ğ‘‡âˆžî€¸ğ‘”(𝑅),𝑋=𝐿,0â‰¤ğ‘…â‰¤ğ‘…ğ‘Ž,𝜕𝑇𝜕𝑅=0,𝑅=0,0≤𝑋≤𝐿,𝐾(𝑇)𝜕𝑇𝜕𝑅=−𝐻(𝑇)ğ‘‡âˆ’ğ‘‡âˆžî€»,𝑅=ğ‘…ğ‘Ž,0≤𝑋≤𝐿.(2.2) Here, ğ‘…ğ‘Ž is radial distance from the center to the surface of the pin fin.

Introducing the dimensionless variables𝜃=ğ‘‡âˆ’ğ‘‡âˆžğ‘‡ğ‘âˆ’ğ‘‡âˆžğ‘‹,𝑥=𝐿𝑅,𝑟=ğ‘…ğ‘Žğ¾,𝑘=ğ¾ğ‘Ž,𝐸2=î‚µğ¿ğ‘…ğ‘Žî‚¶2,𝐿𝑠(𝜃)=2𝑆(𝑇)ğ¾ğ‘Žî€·ğ‘‡ğ‘âˆ’ğ‘‡âˆžî€¸ğ»,ℎ=â„Žğ‘,(2.3) we obtain𝐸21𝑟𝜕𝜕𝑟𝑟𝑘(𝜃)𝜕𝜃+𝜕𝜕𝑟𝜕𝑥𝑘(𝜃)𝜕𝜃𝜕𝑥=𝑠(𝜃),(2.4) and the boundary conditions are𝜕𝜃𝜕𝑥=0,𝑥=0,𝜃=𝑔(𝑟),𝑥=1,𝜕𝜃𝜕𝑟=0,𝑟=0,𝑘(𝜃)𝜕𝜃𝜕𝑟=âˆ’ğµğ‘–â„Ž(𝜃)𝜃,𝑟=1,(2.5) where 𝐸 is the fin extension factor, â„Žğ‘ is the fin base heat transfer coefficient, and 𝐵𝑖 is the Biot number given by â„Žğµğ‘–=ğ‘ğ‘…ğ‘Žğ¾ğ‘Ž.(2.6)

Three physically realistic functions of thermal conductivity are (i) 𝐾 linearly dependent on temperature, (ii) the power law case, and (iii) the exponential case. We focus on two cases: (i) 𝐾(𝑇) depending linearly on temperature; that is, 𝐾(𝑇)=ğ¾ğ‘Žî€·î€·1+ğ›½ğ‘‡âˆ’ğ‘‡âˆžî€¸î€¸,(2.7) and (ii) 𝐾(𝑇) is given by the power law (nonlinear) 𝐾(𝑇)=ğ¾ğ‘Žî‚µğ‘‡âˆ’ğ‘‡âˆžğ‘‡ğ‘âˆ’ğ‘‡âˆžî‚¶ğ‘›.(2.8) In dimensionless variables, we have (i)𝑘(𝜃)=1+𝐵𝜃,(ii)𝑘(𝜃)=𝜃𝑛,(2.9) where 𝐵=𝛽(ğ‘‡ğ‘âˆ’ğ‘‡âˆž). Here, ğ¾ğ‘Ž is the thermal conductivity of the fin at ambient temperature, 𝛽 is the thermal conductivity gradient, 𝑛 is an exponent, and 𝐵 is the thermal conductivity parameter. Applying the Kirchoff's transformation (see, e.g., [16]),𝑤(𝑥,𝑟)=𝜃0𝑘𝜃∗𝑑𝜃∗.(2.10) The boundary value problem reduces to𝐸21𝑟𝜕𝑟𝜕𝑟𝜕𝑤+𝜕𝜕𝑟2𝑤𝜕𝑥2=𝑠(𝑤),(2.11)𝜕𝑤𝑤𝐵𝜕𝑥=0,𝑥=0,(2.12)(1,𝑟)=𝑔(𝑟)+2(𝑔(𝑟))2=𝐹(𝑟),given𝑘=1+𝐵𝜃,(2.13)

or𝑤(1,𝑟)=𝑔(𝑟)𝑛+1𝑛+1=𝐺(𝑟),given𝑘=𝜃𝑛,𝑛≠−1,(2.14)𝜕𝑤𝜕𝑟=0,𝑟=0,(2.15)𝜕𝑤𝜕𝑟=−𝐵𝑖𝑤,𝑟=1,(2.16) where in ğµâ„Ž(𝜃)=1+2𝜃𝜃,when𝑘(𝜃)=1+𝐵𝜃,ℎ(𝜃)=𝑛𝑛+1,when𝑘(𝜃)=𝜃𝑛,𝑛≠−1.(2.17) Note that 𝑤=ln𝜃 when 𝑛=−1 so that (2.4) holds.

3. Classical Lie Point Symmetry Analysis

In brief, a symmetry of a differential equation is an invertible transformation of the dependent and independent variables that leaves the original equation invariant (unchanged). Furthermore, a symmetry of differential equations maps an arbitrary solution to another solution of the same differential equation. Symmetries depend continuously on a parameter and form a group, the one-parameter group of transformations. The classical Lie groups of point invariance transformations act on the system's graph space that is coordinated by the independent and dependent variables. This group may be determined algorithmically (by Lie's classical method), and there are a number of computer algebraic packages developed to construct symmetries (see, e.g., [21–23]), or one may use interactive packages such as REDUCE [24].

Differential equations arising in modelling real-world problems often involve one or more functions depending on either the independent variable or on the dependent variables. It is possible by symmetry techniques to determine the cases which allow the equation in question to admit extra symmetries. The exercise of searching for the forms of arbitrary functions for which extra symmetries are admitted is called group classification. The notion of group classification is pioneered by Lie [25].

The theory and applications of symmetry analysis may be found in excellent text such as those of [26–29]. We adopt the direct methods in [27] (which exclude explicit equivalence transformation analysis) to determine possible forms of the source term for which (2.11) admits extra point symmetries.

In essence, determining classical Lie point symmetries for the governing Equation (2.11) implies seeking transformation of the form𝑟∗=𝑟+𝜖𝜉1𝜖(𝑟,𝑥,𝑤)+𝑂2,𝑥∗=𝑥+𝜖𝜉2𝜖(𝑟,𝑥,𝑤)+𝑂2,𝑤∗𝜖=𝑤+𝜖𝜂(𝑟,𝑥,𝑤)+𝑂2,(3.1) generated by the vector fieldΓ=𝜉1𝜕(𝑟,𝑥,𝑤)𝜕𝑟+𝜉2𝜕(𝑟,𝑥,𝑤)𝜕𝜕𝑥+𝜂(𝑟,𝑥,𝑤),𝜕𝑤(3.2) which leaves the governing equation invariant. Note that we seek symmetries that leave the single (2.11) invariant rather than the entire boundary value problem. This is because the number of symmetries admitted by the governing equation and the imposed boundary conditions is less than for those admitted by the single governing equation. One may apply the boundary condition to the obtained invariant solutions.

The action of Γ is extended to all the derivatives appearing in the governing equation through the second prolongationΓ[2]=Γ+𝜁𝑥𝜕𝜕𝑤𝑥+𝜁𝑟𝜕𝜕𝑤𝑟+𝜁𝑥𝑥𝜕𝜕𝑤𝑥𝑥+𝜁𝑟𝑟𝜕𝜕𝑤𝑟𝑟+⋯,(3.3) where𝜁𝑥=𝐷𝑥(𝜂)−𝑤𝑟𝐷𝑥𝜉1−𝑤𝑥𝐷𝑥𝜉2,𝜁𝑟=𝐷𝑟(𝜂)−𝑤𝑟𝐷𝑟𝜉1−𝑤𝑥𝐷𝑟𝜉2,𝜁𝑥𝑥=𝐷𝑥(𝜁𝑥)−𝑤𝑥𝑟𝐷𝑥𝜉1−𝑤𝑥𝑥𝐷𝑥𝜉2,𝜁𝑟𝑟=𝐷𝑟(𝜁𝑟)−𝑤𝑟𝑟𝐷𝑟𝜉1−𝑤𝑟𝑥𝐷𝑟𝜉2,(3.4) with 𝐷𝑟=𝜕𝜕𝑟+𝑤𝑟𝜕𝜕𝑤+𝑤𝑟𝑟𝜕𝜕𝑤𝑟+𝑤𝑥𝑟𝜕𝜕𝑤𝑥𝐷+⋯,𝑥=𝜕𝜕𝑥+𝑤𝑥𝜕𝜕𝑤+𝑤𝑥𝑥𝜕𝜕𝑤𝑥+𝑤𝑥𝑟𝜕𝜕𝑤𝑟+⋯,(3.5) being the operators of total derivatives. The generator Γ is a Lie point symmetry of (2.11), ifΓ[2](Equation(2.11))∣Equation(2.11)=0.(3.6)

The invariance condition (3.6) yields the determining equations−𝐸21𝑟2𝑤𝑟𝜉1+𝐸21𝑟𝜁𝑟+𝐸2𝜁𝑟𝑟+𝜁𝑥𝑥=ğœ‚ğ‘ î…ž(𝑤),(3.7) on solutions of (2.11). Here prime implies differentiation with respect to 𝑤. Since the coefficient of Γ (the infinitesimals) does not involve the derivatives of the dependent variable, we can separate (3.7) with respect to these derivatives and solve the resulting overdetermined system of linear homogeneous partial differential equations. Further calculations are omitted at this stage since they were facilitated by the freely available interactive computer algebra package REDUCE [24].

In the initial symmetry analysis of (2.11) where 𝑠 is arbitrary, we obtained nothing beyond translation in 𝑥. The cases of the sink or source term for which the principal Lie algebra is extended are listed in Table 1. Wherever they appear in Table 1, ğ‘Ž,𝑏,𝑝, and ğ‘ž are arbitrary constants.


𝑠 ( 𝑤 ) Symmetries

0 Γ 2 = − ( 𝑥 𝜕 𝑥 + 𝑟 𝜕 𝑟 ) , Γ 3 = 𝑤 𝜕 𝑤 − 2 𝑥 𝜕 𝑥 − 2 𝑟 𝜕 𝑟 , Γ 4 = 𝑥 𝑤 𝜕 𝑤 + ( 𝑟 2 − 𝑥 2 ) 𝜕 𝑥 − 2 𝑥 𝑟 𝜕 𝑟 , Γ 5 = ℱ ( 𝑟 , 𝑥 ) 𝜕 𝑤 ,
where ℱ 𝑟 𝑟 + ( ℱ 𝑟 / 𝑟 ) + ℱ 𝑥 𝑥 = 0 .

𝑤 Γ 2 = − 𝑤 𝜕 𝑤 , Γ 3 = ℱ ( 𝑟 , 𝑥 ) 𝜕 𝑤 , where ℱ 𝑟 𝑟 + ℱ 𝑟 / 𝑟 + ℱ 𝑥 𝑥 = 0 .

𝑤 𝑝 , 𝑝 ≠ 5 Γ 2 = 1 / ( 𝑝 − 5 ) ( 2 𝑤 𝜕 𝑤 + ( 1 − 𝑝 ) 𝑥 𝜕 𝑥 + ( 1 − 𝑝 ) 𝑟 𝜕 𝑟 )
𝑝 = 5 Γ 3 = − 𝑥 𝑤 𝜕 𝑤 + ( 𝑥 2 − 𝑟 2 ) 𝜕 𝑥 + 2 𝑥 𝑟 𝜕 𝑟

𝑒 𝑝 𝑤 Γ 2 = ( 1 / 𝑝 ) 𝜕 𝑤 − ( 𝑥 / 2 ) 𝜕 𝑥 − ( 𝑟 / 2 ) 𝜕 𝑟

( ğ‘Ž + 𝑏 𝑤 ) ğ‘ž Γ 2 = 1 / ( ğ‘ž − 5 ) ( ( 2 ( ğ‘Ž + 𝑏 𝑤 ) / 𝑛 ) 𝜕 𝑤 + ( 1 − ğ‘ž / ğ‘ž − 5 ) 𝑥 𝜕 𝑥 + ( ( 1 − ğ‘ž ) / ( ğ‘ž − 5 ) ) 𝑟 𝜕 𝑟 )

ğ‘ž = 5 Γ 3 = − ( 𝑟 ( ğ‘Ž + 𝑏 𝑤 ) / 2 𝑛 ) 𝜕 𝑤 + ( ( 𝑥 2 − 𝑟 2 ) / 2 ) 𝜕 𝑥 + 𝑥 𝑟 𝜕 𝑟

4. Exact Solutions

In this section we construct exact solutions, first using method of separation of variables and secondly using symmetry techniques. Note that 𝑠=0 and 𝑠=𝑤 renders (2.11) linear and hence solvable by method of separation of variable. In fact, the solutions have been constructed, for example, in [16] when 𝑠=0 (source or sink term is neglected).

4.1. Exact Solutions by Separation of Variables

We consider (2.11) with a linear source term. Three cases arise for the separation constant, ğœŽ. Note that ğœŽ=0 leads to trivial solutions.

4.1.1. Case ğœŽ=−𝜆2, 𝜆>0

Exact solution to (2.11) is given by𝑤(𝑥,𝑟)=âˆžî“ğ‘š=1𝑑𝑚𝜆cosh𝑚𝑥𝐽0𝛿𝑚𝑟,(4.1) where eigenvalues 𝜆𝑚 satisfy𝛿𝑚𝐽1𝛿𝑚=−𝐵𝑖𝐽0𝛿𝑚,(4.2) with 𝛿𝑚=𝜆2𝑚−1/𝐸,𝜆2𝑚≠1, for all 𝑚=1,2,3,…, and𝑑𝑚=∫10𝑟𝐹(𝑟)𝐽0𝜆𝑚𝑟𝑑𝑟𝜆cosh𝑚∫10𝑟𝐽20𝜆𝑚𝑟𝑑𝑟,(4.3) given boundary condition (2.13); otherwise, 𝐹(𝑟) may simply be replaced by 𝐺(𝑟) if condition (2.14) is given. Here, 𝐽0 and 𝐽1 are Bessel functions of order 0 and 1, respectively [30]. Solution (4.1) is depicted in Figures 2, 3, 4, 5, 6, 7, 8, and 9. In Figures 2–5, we have plotted solution (4.1) given thermal conductivity which is linearly dependent on temperature, whereas in Figures 6–9, we considered a power law thermal conductivity. Note that for all 𝜆2𝑚=1, we obtain trivial solutions.

4.1.2. Case ğœŽ=𝜆2, 𝜆>0

In this case, we obtain the exact solution𝑤(𝑥,𝑟)=âˆžî“ğ‘š=1𝑐𝑚𝜆cos𝑚𝑥𝐼0𝛼𝑚𝑟,(4.4) where eigenvalues 𝜆𝑚 satisfy𝛼𝑚𝐼1𝛼𝑚=−𝐵𝑖𝐼0𝛼𝑚,(4.5) with 𝛼𝑚=1+𝜆2𝑚/𝐸 and𝑐𝑚=∫10𝑟𝐹(𝑟)𝐼0𝜆𝑚𝑟𝑑𝑟𝜆cos𝑚∫10𝑟𝐼20𝜆𝑚𝑟𝑑𝑟.(4.6) Here, 𝐼0 and 𝐼1 are modified Bessel functions of order 0 and 1, respectively [30]. We omit further analysis of solution 25, since similar observations to solution 24 are obtained. Note that in terms of the original variables, we obtain solutions√𝜃=−1±1+2𝐵𝑤𝐵given𝑘(𝜃)=1+𝐵,𝜃=𝑤1/(𝑛+1)given𝑘(𝜃)=𝜃𝑛,𝑛≠−1,𝜃=𝑒𝑤𝑛=−1.(4.7) with 𝑤 given in Sections 4.1.1 and 4.1.2.

4.2. Symmetry Reductions and Invariant Solutions

If a differential equation is invariant under a Lie point symmetry, then one can reduce the order of the ordinary differential equation or the number of variables of the partial differential equation by one. The reduced equation may or may not be solved exactly. The exact (similarity) solutions obtained via symmetries are referred to as invariant solutions. In this section, we consider two cases as illustrative examples.

4.2.1. Linear Sink Term

We consider the linear combination of the symmetry generators Γ1 and Γ2; namely,Γ1±𝛼1Γ2=𝜕𝜕𝑥±𝛼1𝑤𝜕𝜕𝑤,𝛼1≠0.(4.8)

The basis for the invariants is constructed by the corresponding characteristic equations in Pfaffian form 𝑑𝑤𝑤=±𝛼1𝑑𝑥1=𝑑𝑟0.(4.9) Thus, we obtain the functional form of the solution 𝑤=𝑒±𝛼1𝑥𝑈(𝑟),(4.10) where 𝑈(𝑟) satisfy 𝐸2ğ‘ˆî…žî…ž+𝐸21ğ‘Ÿğ‘ˆî…ž+±𝛼21−1𝑈=0,(4.11) where prime indicates the derivative with respect to 𝑟. The general exact solution to (4.11) is given by 𝑈(𝑟)=ğ‘Ž1𝐽0âŽ›âŽœâŽœâŽœâŽî”Â±ğ›¼21−1ğ¸ğ‘ŸâŽžâŽŸâŽŸâŽŸâŽ +ğ‘Ž2𝑌0âŽ›âŽœâŽœâŽœâŽî”Â±ğ›¼21−1ğ¸ğ‘ŸâŽžâŽŸâŽŸâŽŸâŽ ,(4.12) where ğ‘Ž1 and ğ‘Ž2 are arbitrary constants and 𝐽0 and 𝑌0 are Bessel 𝐽 and 𝑌 functions of order 0, respectively. In terms of the transformed variable 𝑤, we obtain the general exact solution𝑤=ğ‘Ž1𝑒±𝛼1𝑥𝐽0(𝛾𝑟),with𝛾𝐽1(𝛾)+𝐵𝑖𝐽0(𝛾)=0,𝛾=±𝛼21−1𝐸,(4.13) for (2.11) with 𝑠=𝑤. We observe that this solution does not satisfy the boundary conditions at 𝑥=0 and 𝑥=1. One may consider semifinite fins where the temperature gradient vanishes at large 𝑥 values and with a appropriate choice of 𝐹, ğ‘Ž1 may be given by an exponential constant. Note that 𝛼1=1 leads to trivial solutions.

4.2.2. Nonlinear Sink Term

The power law source term 𝑠=𝑤𝑝, 𝑝≠1 renders (2.11) nonlinear and separation of variables is inapplicable. Following the techniques outlined in Section 4.2.1, we observe that the symmetry generator Γ2 listed in Table 1 leads to the reduction𝑤=𝑥2/1−𝑝𝐺𝑥(𝛾),where𝛾=𝑟and𝐺satisfytheO.D.E.(4.14)1+𝐸2𝛾2î€¸ğºî…žî…ž+𝐸24𝛾+11âˆ’ğ‘ğ›¾î‚¼ğºî…ž+221−𝑝11−𝑝−1𝛾21𝐺−𝛾2𝐺𝑝=0,𝑝≠1.(4.15) We observe that (4.15) is harder to solve exactly. Furthermore, the boundary conditions are not invariant under Γ2 given a nonlinear source term.

5. Fin Efficiency and Heat Flux

5.1. Heat Flux

The heat transfer from the fin base may be constructed by evaluating heat conduction rate at the base (see, e.g., [31])ğ‘žğ‘î€œ=2ğœ‹ğ‘…ğ‘Ž0𝐾(𝑇)𝜕𝑇|||𝜕𝑋𝑋=𝐿𝑅𝑑𝑅=2𝜋𝑅2ğ‘Žî€·ğ‘‡ğ‘âˆ’ğ‘‡âˆžî€¸ğ¾ğ‘Žğ¿î€œ10𝑘(𝜃)𝜕𝜃|||𝜕𝑥𝑥=1𝑟𝑑𝑟.(5.1)

The dimensionless heat transfer rate from the base of the fin is defined by [31]ğ‘žğ‘„=𝑏𝐿2ğœ‹ğ¾ğ‘Žî€·ğ‘‡ğ‘âˆ’ğ‘‡âˆžî€¸ğ‘…2ğ‘Ž=10𝑘(𝜃)𝜕𝜃|||𝜕𝑥𝑥=1𝑟𝑑𝑟.(5.2)

5.2. Fin Efficiency

Fin efficiency (overall fin performance) is defined as the ratio of the actual heat transferred from the fin surface to the surrounding fluid to the heat which would be transferred if the entire fin area were kept at the base temperature [2, 32]. For the pin fin, analogous to the definition in [33], the local fin efficiency is defined byğ‘žğœ‚=𝑏𝑄𝑖=2𝜋𝑅2ğ‘Žî€·ğ‘‡ğ‘âˆ’ğ‘‡âˆžî€¸ğ¾ğ‘Žî€¸âˆ«/𝐿10𝑘(𝜃)(𝜕𝜃/𝜕𝑥)∣𝑥=1𝑟𝑑𝑟2ğœ‹ğ‘…ğ‘Žâ„Žğ‘î€·ğ‘‡ğ‘âˆ’ğ‘‡âˆžî€¸ğ¿,(5.3) or simply1𝜂=𝐸2𝐵𝑖10𝑘(𝜃)𝜕𝜃|||𝜕𝑥𝑥=1𝑟𝑑𝑟.(5.4)

5.2.1. Flux and Fin Efficiency Given (4.1)

Given the solution (4.1) with linear thermal conductivity 𝑘=1+𝐵𝜃 as an example, we obtain heat flux for 𝑤𝑄=10𝜕𝑤|||𝜕𝑥𝑥=1𝑟𝑑𝑟=âˆžî“ğ‘š=1𝑑𝑚𝜆𝑚𝜆sinh𝑚𝐽1𝛿𝑚𝛿𝑚,(5.5) and fin efficiency1𝜂=𝐸2𝐵𝑖10𝜕𝑤|||𝜕𝑥𝑥=11𝑟𝑑𝑟=𝐸2ğµğ‘–âˆžî“ğ‘š=1𝑑𝑚𝜆𝑚𝜆sinh𝑚𝐽1𝛿𝑚𝛿𝑚.(5.6)

6. Entropy Generation Analysis

Entropy generation results from the nonequilibrium conditions arising due to the exchange of energy within the fluid (in case of a flow between two plates) and the solid boundaries [34]. In fact, entropy generation analysis has been limited to vertical cylindrical annulus (or channels) (see, e.g., [35–37]), and studies in pure conduction may be found in the literature such as in [38–40]. The local volumetric rate of entropy generation is given in dimensionless variable (see, e.g., [17])𝑁𝐿=𝜕𝜃𝜕𝑟2+𝜕𝜃𝜕𝑥2.(6.1) The total dimensionless entropy generated in a pin fin is given by [17]𝑁𝑇=10𝜕𝜃𝜕𝑟2+𝜕𝜃𝜕𝑥2𝑟𝑑𝑟𝑑𝑥.(6.2) Given 𝑘=1+𝐵𝜃, we have in terms of 𝑤𝑁𝐿=11+2𝐵𝑤𝜕𝑤𝜕𝑟2+𝜕𝑤𝜕𝑥2,𝑁𝑇=1011+2𝐵𝑤𝜕𝑤𝜕𝑟2+𝜕𝑤𝜕𝑥2𝑟𝑑𝑟𝑑𝑥.(6.3)

7. Discussions

We follow the analysis in [17]. The number of eigenvalues required to calculate the temperature distribution, heat flux, and fin efficiency accurately depend on the Biot number 𝐵𝑖. We observe in Table 2 below that Biot number is inversely proportional to the eigenvalues. The expression for the temperature distribution is given explicitly in (4.1) and (4.4). However, in further analysis, we focus on solution (4.4). The temperature distribution depends on a number of variables including 𝐵𝑖, eigenvalues, and the arbitrary function of 𝑟 describing the temperature at the base of the fin. We may choose any function 𝑔 such that ğ‘”î…ž(0)=0. In fact, the nonuniform base temperature is modeled by cosine function of 𝑟, namely, 1+𝑝cos𝑟 for some parameter 𝑝 [13], and base temperature may be given in general [41] by the power law 1+𝑝cos𝜅𝑟, 𝜅 being an exponent (see also Chapter 15 in [1]). In Figure 2, not surprisingly, we observe that the temperature is higher at the center of the pin, that is, at 𝑟=0. Figure 3 depicts the temperature profile along the 𝑟=0, and temperature decreases from the base to the tip of the fin. We observe in Figures 4 and 5 that the temperature is much higher at the center of the pin than at its surface. Similar results are recorded in the literature (see, e.g., [17]). Similar profiles are observed in Figures 6–9, wherein thermal conductivity is assumed to be given by the power law. We note the difference at surface of the fin tip in Figures 4 and 9. In both cases, the temperature drops even to the negative values when 𝑘 is linear in temperature. The drop in the temperature is due to the presence of the sink term.


𝐵 𝑖 0.2 0.4 0.6 0.8 1 2

𝜆 1 7.6243 7.5193 7.4141 7.3093 7.2056 6.7249
𝜆 2 14.0098 13.9527 13.8955 13.8384 13.7815 13.5023
𝜆 3 20.3322 20.2928 20.2535 20.2141 20.1748 19.9801
𝜆 4 26.6361 26.6060 26.5760 26.5460 26.5160 26.3667
𝜆 5 32.9322 32.9079 32.8836 32.8593 32.8350 32.7140
𝜆 6 39.2241 39.2037 39.1833 39.1629 39.1425 39.0408
𝜆 7 45.5136 45.4960 45.4784 45.4608 45.4433 45.3556
𝜆 8 51.8016 51.7861 51.7707 51.7552 51.7398 51.6627
𝜆 9 58.0885 58.0747 58.0609 58.0472 58.0334 57.9646
𝜆 1 0 64.3747 64.3623 64.3498 64.3374 64.3250 64.2629

The classical Lie point symmetry analysis resulted in a number of admitted symmetries. In general, symmetries yield self-similar or similarity solutions known also as invariant solutions. It is more difficult to construct invariant (similarity) solutions for the boundary value problem defined by characteristic length. However, one may consider the semiinfinite fins (see also [1]), whereby either temperature or temperature gradient vanishes at large spatial variable. In our case, at large 𝑥. Note that construction of invariant solutions for steady nonlinear one-dimensional problems is easier (see, e.g., [6]). On the other hand, symmetry techniques may be use to reduce the boundary value problem in partial differential equation to the boundary value problem in ordinary differential equations, as such the reduced problem may be solve exactly or easily by numerical schemes.

8. Concluding Remarks

We have considered a steady state problem describing heat dissipation in a pin fin. We have successfully applied the Kirchoff transformation to partly linearize the resulting nonlinear diffusion equation. To the best of our knowledge, symmetry methods have not yet been applied to two-dimensional fin problems. Some cases of the source term for which the governing equation admits extra symmetries have been obtained. Unfortunately, admitted symmetries do not leave the entire boundary value problem invariant. Some new solutions are constructed by separation of variables. Heat transfer analysis is carried out following the work in [17]. Further analysis into the influence of a larger number of terms may reveal a more in depth understanding of the underlying dynamics of the system under consideration.

Acknowledgments

R. J. Moitsheki wishes to thank the National Research Foundation of South Africa under Thuthuka program for the continued generous financial support. The authors thank the anonymous referees on pointing out a number of references and for the valuable comments which led to clarifications and improvements to this paper.

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Copyright © 2011 Raseelo J. Moitsheki and Charis Harley. This is an open access article distributed under the Creative Commons Attribution License, which permits unrestricted use, distribution, and reproduction in any medium, provided the original work is properly cited.


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