# A High Order Theory for Linear Thermoelastic Shells: Comparison with Classical Theories

Authors: V. V. Zozulya
Journal: Journal of Engineering
 (2013)

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## Abstract

A high order theory for linear thermoelasticity and heat conductivity of shells has been developed. The proposed theory is based on expansion of the 3-D equations of theory of thermoelasticity and heat conductivity into Fourier series in terms of Legendre polynomials. The first physical quantities that describe thermodynamic state have been expanded into Fourier series in terms of Legendre polynomials with respect to a thickness coordinate. Thereby all equations of elasticity and heat conductivity including generalized Hooke's and Fourier's laws have been transformed to the corresponding equations for coefficients of the polynomial expansion. Then in the same way as in the 3D theories system of differential equations in terms of displacements and boundary conditions for Fourier coefficients has been obtained. First approximation theory is considered in more detail. The obtained equations for the first approximation theory are compared with the corresponding equations for Timoshenko's and Kirchhoff-Love's theories. Special case of plates and cylindrical shell is also considered, and corresponding equations in displacements are presented.


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## Body

## 1. Introduction

The development of microelectromechanical and nanoelectromechanical technologies extends the field of application of the classical or nonclassical theories of plates and shells towards the new thin-walled structures. The classical elasticity can be extended to the micro- and nanoscale by implementation of the theory of elasticity taking into account the physical phenomenon that can occur in such structures and devices [1, 2].Classical theories of beams, rods, plates, and shells are usually related to names of Bernoulli, Euler, Kirchhoff, and Love. These theories are based on well-known physical hypothesis; they are very popular among an engineering community because of their relative simplicity and physical clarity. Numerous books and monographs have been written in the subject among others one can refer to [3–6]. But unfortunately classical theories have some shortcomings and logical contradictions such as their proximity and inaccuracy and as result in some cases not good agreement with results obtained with 3D approach and experiments. Therefore there is demand in developing new more accurate theories.We can mention at least two approaches to development of the theories of thin-walled structures.  One consists in improvement of the classical physical hypothesis and development of more accurate theories. The theory of beamis well-known model that takes into account transversal deformations developed by Timoshenko and extended to the plate theory by Mindlin [7]. This theory was extended and applied to shells of arbitrary geometry in numerous publications and is referred to as Timoshenko’s theory that takes into account in-plane shear deformations and rotation of the elements perpendicular to the middle surface of the shell [8–10].The second approach consists in expansion of the stress-strain field components into polynomials series in terms of thickness. It was proposed by Cauchy and Poisson and at that time was not popular. Significant  extension and development of that method were done by Kil'chevskii [11]. Vekua has used Legendre’s polynomials for the expansion of the equations of elasticity and reduction of the 3-D problem to 2-D one [12]. Such an approach has significant advantages because Legendre’s polynomials are orthogonal, and as a result obtained equations are simpler. This approach was extended and applied to dynamical problems [13], thermoelasticity [14], and composite and laminate shells [15].The approach developed in [12–15] has been applied to the plates and shells thermoelastic contact problems when mechanical and thermal conditions are changed during deformation in our previous publications [16–29]. The mathematical formulation, differential equations, and contact conditions for the cases of plates and cylindrical shells for the first time have been reported in [16–18]. In more general form with extension to nonstationary processes and calculation of all coefficients of the equations and contact and boundary conditions it was presented in [19, 20]. Then the approach was further developed to contact of plates and shells with rigid bodies through heat conducting layer [21–25], thermoelasticity of the laminated composite materials with possibility of delamination and mechanical and thermal contact in temperature field in [21, 22, 26], the pencil-thin nuclear fuel rods modeling in [22], and functionally graded shells in [28, 29].Bibliography related to different aspects of the theory and applications of the thin-walled structures contains of several thousands publications for references one can see review papers [30, 31]. For trends and recent development in the shells theory and its applications one can refer to books [10, 32–34].In this paper, an approach based on expansion of the equations of thermoelasticity and heat conductivity into Fourier series in terms of Legendre polynomials has been developed and applied to high order theory of arbitrary geometry shells. For that purpose we expand functions that describe thermodynamic state of elastic body into Fourier series in terms of Legendre polynomials with respect to thickness and find corresponding relations of thermoelasticity and heat conductivity for Fourier coefficients of those. Then using techniques developed in our previous publications we find system of differential equations and boundary conditions for Fourier coefficients. Case of first approximation (Vekua’s) theory is considered in more detail, and all relations and equations are explicitly presented. Obtained equations for Vekua’s shell theory have been analyzed and compared with classical Timoshenko’s and Kirchhoff-Love's shell theories.


## 2.3-D Formulation

Let an elastic body occupy an open 3-D Euclidian space in simply connected bounded domainV∈R3 with a smooth boundary ∂V. We assume that body is homogeneous isotropic shell of arbitrary geometry with 2h thickness, material of which follows linear physical laws of thermoelasticity and heat conductivity. The shell occupies the domain V=Ω×[-h,h] in Euclidean space. Boundary of the shell can be presented in the form ∂V=S∪Ω+∪Ω-. Here Ω is the middle surface of the shell, ∂Ω is its boundary, Ω+ and Ω- are the outer sides, and S=∂Ω×[-h,h] is a sheer side.Thermodynamic state of the body is defined by stressσij(x,t) and strain εij(x,t) tensors and displacements ui(x,t), traction pi(x,t), and body forces bi(x,t) vectors, temperature θ(x,t),  and vector of thermal flow qi(x,t) and specific strength of the internal heat sources χ(x,t), respectively. These quantities are not independent they are related by equations of linear thermoelasticity and heat conductivity.We introduce orthogonal system of coordinatesx1,x2, and x3, such that position vector of arbitrary point is equal to R(x1,x2,x3)=eixi. Unit orthogonal basic vectors and their derivatives with respect to space coordinates are equal to
(1)ei=1Hi∂R∂xi,∂ei∂xj=Γijkek,
where Hi are Lame coefficients and Γijk are  Christoffel symbols. They are calculated by the equations
(2)Hi=|∂R∂xi|=∂R∂xi·∂R∂xi,Γijk=-1Hi∂Hi∂xjδik+12HiHk×(δjk∂HjHk∂xi+δik∂HiHk∂xj-δij∂HiHj∂xk).
From the last equation it follows that Γijk=0 for i≠j≠k and
(3)Γiik=-1Hk∂Hi∂xk,Γikk=-1Hi∂Hk∂xifori≠k.In the case if displacements and their gradients are small, the following kinematic Cauchy relations take place:(4)εij=12(1Hj∂ui∂xj+1Hi∂uj∂xi)+Γijkuk.Equations of motion have the form(5)1Hj∂σij∂xj+σijHkΓikk+σikHiΓkij+bi=ρu¨i,
where upper points are partial derivatives with respect to time t.We assume that the stressσij(x) and deformation εij(x) tensors and temperature θ(x,t) are related by equations
(6)σij=cijklσkl+βijθ,cijkl=cjikl=cklij,βij=βji,
where cijkl and βij are elastic modulus and the coefficients of linear thermal expansion. In the isotropic case
(7)cijkl=λδijδkl+μ(δikδjl+δilδkj),βij=βTδij,
where λ and μ are the Lame constants, βT=(μ+3λ)αT, and αT is a coefficient of linear thermal expansion.Equations (6) and (7) are referred to as generalized Hooke’s law. They were introduced by Duhamel and substantiated using thermodynamic methods by Bio [8, 11].Heat is distributed in the body according to Fourie’s law:(8)qi=λij1Hj∂θ∂xj,
where λij is the tensor of coefficients of thermal conductivity of the body, in the isotropic case λij=δijλT, and λT is the coefficient of thermal conductivity of the body.For convenience we transform the previous equations taking into account that the position vectorR(x) of any point in domain V, occupied by material points of shell, may be presented as
(9)R(x)=r(xα)+x3n(xα),
where r(xα) is the position vector of the points located on the middle surface of shell and  n(xα) is a unit vector normal to the  middle  surface.We consider thatxα=(x1,x2) are curvilinear coordinates associated with main curvatures of the middle surface of the shell. In this case 3-D equations (4)–(8) can be simplified taking into account that Lame coefficients and their derivatives have the form
(10)Hα=Aα(1+kαx3)forα=1,2,H3=1∂Hβ∂xα=∂Aβ∂xα(1+kαx3),∂Hβ∂x3=kβAβ,∂H3∂xi=0.The equations of motion (5) after simplification have the form
(11)∂(A2σ11)∂x1+∂(A1σ12)∂x2+A1A2∂σ13∂x3+σ12∂A1∂x2+σ13A1A2k1-σ22∂A2∂x1+A1A2b1=ρA1A2u¨1,∂(A2σ21)∂x1+∂(A1σ22)∂x2+A1A2∂σ23∂x3+σ21∂A2∂x1+σ23A1A2k2-σ11∂A1∂x2+A1A2b2=ρA1A2u¨2,∂(A2σ31)∂x1+∂(A1σ32)∂x2+∂(A1A2σ33)∂x3-σ11A1A2k1-σ22A1A2k2+A1A2b3=ρA1A2u¨3.The kinematic Cauchy relations (4) have the form
(12)ε11=1A1∂u1∂x1+1A1A2∂A1∂x2u2+k1u3,ε22=1A2∂u2∂x2+1A2A1∂A2∂x1u1+k2u3,ε33=∂u3∂x3,ε12=1A2(∂u1∂x2-1A1∂A2∂x1u2)+1A1(∂u2∂x1-1A2∂A1∂x2u1),ε13=∂u1∂x3-k1u1+1A1∂u3∂x1,ε23=∂u2∂x3-k2u2+1A2∂u3∂x2.
In (10)–(12), Aα(x1,x2)=(∂r(x1,x2))/∂xα are coefficients of the first quadratic form of a surface, and kα(x1,x2) are its main curvatures. We also take into account that shell is relatively thin, and therefore
(13)1Hα∂Hβ∂xα=1Aα∂Aβ∂xα,1+kαx3≈1→Hα≈Aα.Following [8, 11] we can present coupled system of the equations of linear thermoelasticity and heat conductivity in the form
(14)L·u+βT∇θ+b=ρu¨,∀x∈V,∀t∈ℑ=[0,T],λTΔθ-χ=cεθ˙+βTθ0(∇·u˙).The differential operatorL=Lijei⊗ej for homogeneous isotropic medium has the form
(15)L·u=μΔu+(λ+μ)∇(∇·u).
Other differential operators presented in (14) and (15), respectively, in the system of coordinates introduced here related to middle surface of the shell have the form
(16)∇(u)1=1A1∂u1∂x1+1A2∂u1∂x2+∂u1∂x3,∇(∇·u)α=1Aα∂∂xα(1A1A2[∂(A2u1)∂x1+∂(A1u2)∂x2]+∂u3∂x3+(k1+k2)u31A1A2),∇(∇·u)3=∂∂x3(1A1A2[∂(A2u1)∂x1+∂(A1u2)∂x2]+∂u3∂x3+(k1+k2)u31A1A2),∇θ=1A1∂θ∂x1+1A2∂θ∂x2+∂θ∂x3.For mathematically correct formulation of the coupled problem of thermoelasticity and heat conductivity we have to formulate initial and boundary conditions. Initial conditions consist of assignment of the displacements, velocity, and temperature distribution in the initial moment of time. They can be written in the form(17)ui(x,0)=ui0(x),∂tui(x,0)=vi0(x),θ(x,0)=θ0(x).If the body occupied a finite regionV with the boundary ∂V, it is necessary to assign boundary conditions. We consider the mixed boundary conditions in the form
(18)ui(x,t)=uib(x,t),∀x∈∂Vu,∀t∈ℑ,pi(x,t)=σij(x,t)nj(x)=pib(x,t),∀x∈∂Vp,∀t∈ℑ,θ(x,t)=θb(x,t),∀x∈∂Vθ,∀t∈ℑ,qi(x,t)=qib(x,t),∀x∈∂Vq,∀t∈ℑ.Now we can transform 3-D equations of thermoelasticity and heat conductivity in 2-D equations using Legendre polynomials series expansion.


## 3.2-D Formulation

We expand the physical parameters, that describe the thermodynamic state of the body, into the Legendre polynomials series along the coordinatex3. Such expansion can be done because any function f(p), which is defined in domain -1≤p≤1 and satisfies Dirichlet’s conditions (continuous, monotonous, and having finite set of discontinuity points), can be expanded into Legendre’s series according to formulas
(19)f(p)=∑k=0∞akPk(p)wherean=2k+12∫-11f(p)Pk(p)dp.
Any function of more than one independent variable can also be expanded into Legendre’s series with respect to for example, variable x3∈[-1,1], but first the new normalized variable ω=x3/h∈[-1,1] has to be introduced. Taking into account (19) we have
(20)ui(x,t)=∑k=0∞uik(xα,t)Pk(ω),σij(x,t)=∑k=0∞σijk(xα,t)Pk(ω),εij(x,t)=∑k=0∞εijk(xα,t)Pk(ω),θ(x,t)=∑k=0∞θk(xα,t)Pk(ω),(21)uik(xα,t)=2k+12h∫-hhui(xα,x3,t)Pk(ω)dx3,σijk(xα,t)=2k+12h∫-hhσij(xα,x3,t)Pk(ω)dx3,εijk(xα,t)=2k+12h∫-hhεij(xα,x3,t)Pk(ω)dx3,θk(xα,t)=2k+12h∫-hhθ(xα,x3,t)Pk(ω)dx3.
The following relations take place for the derivatives with respect to time:
(22)2k+12h∫-hh∂tui(xα,x3,t)Pk(ω)dx3=∂tuik(xα,t),2k+12h∫-hh∂t2ui(xα,x3,t)Pk(ω)dx3=∂t2uik(xα,t),2k+12h∫-hh∂tθ(xα,x3,t)Pk(ω)dx3=∂tθk(xα,t),
and for the derivatives with respect to coordinates xα:
(23)2k+12h∫-hh∂ui(xα,x3,t)∂xαPk(ω)dx3=∂uik(xα,t)∂xα,2k+12h∫-hh∂σij(xα,x3,t)∂xαPk(ω)dx3=∂σijk(xα,t)∂xα,2k+12h∫-hh∂θ(xα,x3,t)∂xαPk(ω)dx3=∂uik(xα,t)∂xα,
respectively.Integration of the derivatives with respect to coordinatesx3 gives us
(24)2k+12h∫-hh∂ui(x,t)∂x3Pk(ω)dx3=uik_(xα,t),2k+12h∫-hh∂σi3(x,t)∂x3Pk(ω)dx3=2k+1h[σi3+(xα,t)-(-1)kσi3-(xα,t)]-σi3k_(xα,t),2k+12h∫-hh∂3θ(x,t)Pk(ω)dx3=∂3θ(xα,t)=Q3k(xα,t),2k+12h∫-hh∂32θ(x,t)Pk(ω)dx3=2k+1h[Q3+(xα,t)-(-1)kQ3-(xα,t)]+Q3k_(xα,t),
where
(25)uik_(xα,t)=2k+1h(uik+1(xα,t)+uik+3(xα,t)+⋯),σi3k_(xα,t)=A1A22k+1h(σi3k-1(xα,t)+σi3k-3(xα,t)+⋯),Q3k_(xα,t)=-A1A22k+1h(Q3k-1(xα,t)+Q3k-3(xα,t)+⋯).Now substituting stress tensor from (20) with considering the equations of motion (11), multiplying obtained relations by Pk(ω), and integrating over interval [-h,h] with respect to x3 we obtain 2-D equations of motion in the form
(26)∂(A2σ11k)∂x1+∂(A1σ12k)∂x2+σ12k∂A1∂x2+σ13kA1A2k1-σ22k∂A2∂x1-σ13k_+A1A2f1k=ρA1A2∂t2u1k,∂(A2σ21k)∂x1+∂(A1σ22k)∂x2+σ12k∂A2∂x1+σ23kA1A2k2-σ11k∂A2∂x1-σ23k_+A1A2f2k=ρA1A2∂t2u2k,∂(A2σ31k)∂x1+∂(A1σ32k)∂x2-σ11kA1A2k1-σ22kA1A2k2-σ33k_+A1A2f3k=ρA1A2∂t2u3k,
where
(27)fik(xα)=bik(xα)+2k+1h(σi3+(xα)-(-1)kσi3-(xα)).In the same way the 2-D kinematic Cauchy relations can be found:(28)ε11k=1A1∂u1k∂x1+1A1A2∂A1∂x2u2k+k1u3k,ε22k=1A2∂u2k∂x2+1A1A2∂A2∂x1u1k+k2u3k,ε12k=1A2(∂u1k∂x2-1A1∂A2∂x1u2k)+1A1(∂u2k∂x1-1A2∂A1∂x2u1k),ε13k=1A1∂u3k∂x1-k1u1k+u1k_,ε23k=1A2∂u3k∂x2-k2u2k+u2k_,ε33=u3k_.
Let us consider generalized Hooke’s law for homogeneous anisotropic body
(29)σijk=cijklεklk+βijθk
and for isotropic one
(30)σ11k=(λ+2μ)ε11k+λ(ε22k+ε33k)+βTθk,σ22k=(λ+2μ)ε22k+λ(ε11k+ε33k)+βTθk,σ33k=(λ+2μ)ε22k+λ(ε11k+ε22k)+βTθk,σ12k=με12k,σ13k=με13k,σ23k=με23k.
In the previously mentioned relations (26)–(30) the following orthogonality property of the Legendre’s polynomials has been used:
(31)∫-hhPn(ω)Pm(ω)dx3={2h2n+1forn=m0forn≠m.In order to find 2-D differential equations in the form of displacements we substitute the kinematic Cauchy relations (28) with Hooke’s law for homogeneous body (30). As a result we have
(32)σ11k=(λ+2μ)(1A1∂u1k∂x1+1A1A2∂A1∂x2u2k+k1u3k)+λ(1A2∂u2k∂x2+1A1A2∂A2∂x1u1k+k2u3k+u3k_)+βTθk,σ22k=(λ+2μ)(1A2∂u2k∂x2+1A1A2∂A2∂x1u1k+k2u3k)+λ(1A1∂u1k∂x1+1A1A2∂A1∂x2u2k+k1u3k+u3k_)+βTθk,σ33k=(λ+2μ)u3k_+λ((1A1∂u1k∂x1+1A1A2∂A1∂x2u2k+k1u3k)+(1A2∂u2k∂x2+1A1A2∂A2∂x1u1k))+βTθk,σ12k=μ(1A2(∂u1k∂x2-1A1∂A2∂x1u2k)+1A1(∂u2k∂x1-1A2∂A1∂x2u1k)),σ13k=μ(1A1∂u3k∂x1-k1u1k+u1k_),σ23k=μ(1A2∂u3k∂x2-k2u2k+u2k_).Substitution of these equations in the equations of equilibrium (26) gives us the 2-D equations in displacements in the form
(33)∑l=0∞Lijklujl-σi3k_+Likθk+A1A2fik=ρA1A2u¨ik,λTΔθk+Q3k__+χk=cεθ˙k+βTθ0[∇·u˙k+2k+1h(u˙3k+1+u˙3k+3⋯)],
where
(34)Q3k__=2k+12h[Q3+-(-1)kQ3-]-1A1A2Q3k_+(k1+k2)Q3k.Now instead of the finite 3-D system of the differential equations in displacements (14) we have an infinite system of 2-D differential equations for coefficients of the Legendre’s polynomial series expansion.  In order to simplify the problem approximate theory has to be developed, and only the finite number of members has to be taken into account in the expansion (20) and in all the previous relations. For example, if we consider n-order approximate shell theory, only n+1 members in the expansion (20) are taken into account:
(35)ui(x,t)=∑k=0nuik(xα,t)Pk(ω),σij(x,t)=∑k=0nσijk(xα,t)Pk(ω),εij(x,t)=∑k=0nεijk(xα,t)Pk(ω),θ(x,t)=∑k=0nθk(xα,t)Pk(ω).
In this case we consider that uik=0,σijk=0,εijk=0 and θk=0 for k<0 and for k>n.Order of the system of differential equations depends on assumption regarding thickness distribution of the stress-strain parameters of the shell.


## 4. Vekua’s Shell Equations

In the case if only the first two terms of the Legendre polynomials series are considered in the expansion (20) we have the first approximation shell theory which is usually referred to as Vekua’s shell theory. In this case the thermodynamic parameters, which describe the state of the shell, can be presented in the form
(36)σij(x,t)=σij0(xα,t)P0(ω)+σij1(xα,t)P1(ω),ui(x,t)=ui0(xα,t)P0(ω)+ui1(xν,t)P1(ω),εij(x,t)=εij0(xα,t)P0(ω)+εij1(xα,t)P1(ω),θ(x,t)=θ0(xα,t)P0(ω)+θ1(xα,t)P1(ω),
where coefficients of the expansion are
(37)ui0(xα,t)=12h∫-hhui(xα,x3,t)dx3,ui1(xα,t)=32h∫-hhui(xα,x3,t)x3dx3,εij0(xα,t)=12h∫-hhεij(xα,x3,t)dx3,εij1(xα,t)=32h∫-hhεij(xα,x3,t)x3dx3,σij0(xα,t)=12h∫-hhσij(xα,x3,t)dx3,σij1(xα,t)=32h∫-hhσij(xα,x3,t)x3dx3,θ0(xα,t)=12h∫-hhθ(xα,x3,t)dx3,θ1(xα,t)=32h∫-hhθ(xα,x3,t)x3dx3.
The equations of motion (26) in this case have the form
(38)∂(A2σ110)∂x1+∂(A1σ120)∂x2+σ120∂A1∂x2+σ130A1A2k1-σ220∂A2∂x1-σ130_+A1A2f10=ρA1A2u¨10,∂(A2σ210)∂x1+∂(A1σ220)∂x2+σ120∂A2∂x1+σ230A1A2k2-σ110∂A2∂x1-σ230_+A1A2f20=ρA1A2u¨20,∂(A2σ310)∂x1+∂(A1σ320)∂x2-σ110A1A2k1-σ220A1A2k2-σ330_+A1A2f30=ρA1A2u¨30,∂(A2σ111)∂x1+∂(A1σ121)∂x2+σ121∂A1∂x2+σ131A1A2k1-σ221∂A2∂x1-σ131_+A1A2f11=ρA1A2u¨11,∂(A2σ211)∂x1+∂(A1σ221)∂x2+σ121∂A2∂x1+σ231A1A2k2-σ111∂A2∂x1-σ231_+A1A2f21=ρA1A2u¨21,∂(A2σ311)∂x1+∂(A1σ321)∂x2-σ111A1A2k1-σ221A1A2k2-σ331_+A1A2f31=ρA1A2u¨31.
The kinematic Cauchy relations (28) have the form
(39)ε110=1A1∂u10∂x1+1A1A2∂A1∂x2u20+k1u30,ε220=1A2∂u20∂x2+1A1A2∂A2∂x1u10+k2u30,ε120=1A2(∂u10∂x2-1A1∂A2∂x1u20)+1A1(∂u20∂x1-1A2∂A1∂x2u10),ε130=1A1∂u30∂x1-k1u10+1hu11,ε230=1A2∂u30∂x2-k2u20+1hu21,ε330=1hu31,ε111=1A1∂u11∂x1+1A1A2∂A1∂x2u21+k1u31,ε221=1A2∂u21∂x2+1A1A2∂A2∂x1u11+k2u31,ε121=1A2(∂u11∂x2-1A1∂A2∂x1u21)+1A1(∂u21∂x1-1A2∂A1∂x2u11),ε131=1A1∂u31∂x1-k1u11,ε231=1A2∂u31∂x2-k2u21,ε331=0.
The generalized Hooke’s law for homogeneous isotropic material (30) has the form
(40)σ110=(λ+2μ)ε110+λ(ε220+ε330)+βTθ0,σ220=(λ+2μ)ε220+λ(ε110+ε330)+βTθ0,σ330=(λ+2μ)ε220+λ(ε110+ε220)+βTθ0,σ120=με120,σ130=με130,σ230=με230,σ111=(λ+2μ)ε111+λ(ε221+ε331)+βTθ1,σ221=(λ+2μ)ε221+λ(ε111+ε331)+βTθ1,σ331=(λ+2μ)ε221+λ(ε111+ε221)+βTθ1,σ121=με121,σ131=με131,σ231=με231.Substitution of the kinematic Cauchy relations (39) with the generalized Hooke’s law (40) and the result of the equations of motion (38) give us the 2-D equations in displacements for Vekua’s shell theory in the form
(41)Lij00uj0+Lij01uj1+Li0θ0+A1A2bik=ρA1A2u¨ik,Lij10uj0+Lij11uj1+Li1θ1+A1A2bik=ρA1A2u¨ik,
and the equation of heat conductivity  in the form
(42)λTΔθ0+Q30__+χ0=cεθ˙0+βτθ0(∇·u˙0+1hu˙31),λTΔθ1+Q31__+χ1=cεθ˙1+βτθ0∇·u˙1,
where Q3+,Q3-,Q30, and Q31 depend on thermal conditions on the outer sides Ω+ and Ω- of the shell. In the case if temperatures  θ+ and θ- are prescribed on Ω+ and Ω-, respectively, they have the form
(43)Q3+-Q3-=34h(θ++θ-)+3θ02h,Q30=12h(θ+-θ-),Q3++Q3-=32h(θ+-θ-)-5θ12h,Q31=32h(θ++θ-)-3θ12h.Differential operators that appear in the equations of thermoelasticity (41) and heat conductivity (42) for shells of arbitrary geometry are presented in the Appendix Section.


## 5. Timoshenko’s Shell Equations

Timoshenko's theory of shells is based on assumptions concerning the value and distribution of the stress-strain state of the shell. Thus, according to static assumptionsσ33=0 and according to kinematic assumptions ε33=0. In this theory the thermodynamic state of shells is determined by quantities specified on the middle surface. The stress state is characterized by the normal nαα, tangential nαβ(α≠β), and shear nα3 forces, as well as the bending mαα and twisting mαβ(α≠β) moments. They are defined as follows:
(44)nαβ=∫-hhσαβdx3,n3β=∫-hhσ3βdx3,mαβ=∫-hhσαβx3dx3.
Comparison with (37) gives us the following relation between corresponding parameters in Vekua’s and Timoshenko’s theories:
(45)σiβ0~niβ2h,σαβ1~3mαβ2h2.
Components σ330 and σ331 are not taken into account in Timoshenko's theory of shells. That follows also from the static hypothesis.Displacements in the Timoshenko's theory of shells are defined by vectorsu(xα,t) and γ(xα,t) with components ui,i=1,2,3 and γα,α=1,2, respectively.  They correspond to displacements of the middle surface and rotation of the elements perpendicular to the middle surface in the planes (xα,x3). These parameters are related to the coefficients of the displacements expansion in the Vekua’s theory in the following way:
(46)ui0~ui,uα1~γαh.
Component u31 is not taken into account in Timoshenko's theory of shells.Deformations in Timoshenko’s theory are determined by the relations(47)εαβ=eαβ+καβx3,εα3=eα3.
Roughly speaking components eαβ correspond to the tension-compression deformation of the middle surface, components eα3 to the transversal shear deformation, and components καβ to the bending and twisting middle surface, respectively. The following formulas give us relations with corresponding quantities in Vekua’s theory:
(48)εαi0~eαi,εαβ1~καβ.
Component ε330 and ε331 are not taken into account in the Timoshenko's theory of shells. That follows also from the kinematic hypothesis.The kinematic Cauchy relations in Timoshenko's theory of shells have the following form:(49)e11=1A1∂u1∂x1+1A1A2∂A1∂x2u2+k1u3,e22=1A2∂u2∂x2+1A1A2∂A2∂x1u1+k2u3,e12=1A2(∂u1∂x2-1A1∂A2∂x1u2)+1A1(∂u2∂x1-1A2∂A1∂x2u1),e13=1A1∂u3∂x1-k1u1+1hγ1,ε230=1A2∂u3∂x2-k2u2+1hγ2,ε330=0,κ11=1A1∂γ1∂x1+1A1A2∂A1∂x2γ2,κ22=1A2∂γ2∂x2+1A1A2∂A2∂x1γ1,κ12=1A1∂γ2∂x1-1A1A2∂A1∂x2γ1+k1ω2,κ21=1A2∂γ1∂x2-1A1A2∂A2∂x1γ2+k2ω1,ω1=1A1∂u2∂x1-1A1A2∂A1∂x2u1,ω2=1A2∂u1∂x2-1A1A2∂A2∂x1u2.The equations of motion have the form(50)∂(A2n11)∂x1+∂(A1n12)∂x2+n12∂A1∂x2-n22∂A2∂x1+n13A1A2k1+A1A2f1k=ρA1A2u¨1,∂(A2n12)∂x1+∂(A1n22)∂x2+n21∂A2∂x1-n11∂A2∂x1+n23A1A2k2+A1A2f2k=ρA1A2u¨2,∂(A2n31)∂x1+∂(A1n32)∂x2-n11A1A2k1-n22A1A2k2+A1A2f3k=ρA1A2u¨3,∂(A2m11)∂x1+∂(A1m12)∂x2+m12∂A1∂x2-m22∂A2∂x1-n13A1A2=ρA1A2hγ¨1,∂(A2m21)∂x1+∂(A1m22)∂x2+m21∂A2∂x1-m11∂A2∂x1-n23A1A2=ρA1A2hγ¨2,n12+m12k1=n21+m21k2.The generalized Hooke’s law for Timoshenko's theory of shells has the form(51)nαα=2Eh1-υ2[eαα+υeββ-(1+υ)αTθ0],n12=Eh1+υe12,nα3=Eh1+υeα3,mαα=2Eh1-υ2[καα+υκββ-(1+υ)αTθ1].m12=2Eh33(1+υ)e12.
Such form of the generalized Hooke’s law follows from the static hypothesis according to which σ33=0, and therefore
(52)ε33=-υ1-υ(ε11+ε22).Substituting kinematic relations (49) with generalized Hooke’s law (51) and considering the result of the equations of motion (50) we obtain the following system of the differential equations in the form of displacements:
(53)Lij00uj+Liβ01γβ+Li0θ0+A1A2bi=ρA1A2u¨i,Lαj10uj+Lαβ11γβ+Lα1θ1+A1A2mα=ρA1A2hγ¨α.Differential operators that appear in (53) for shells of arbitrary geometry are presented in the Appendix Section.The equations of heat conductivity in Timoshenko's theory of shells have the same form as in the Vekua’s shells theory, that is, defined by (42).Components of the stress tensor can be calculated from the equations(54)σαβ(x)=nαβ(xα)2h+3mαβ(xα)x3h3,σα3(x)=nα3(xα)2h,σ33(x)=0.The equations presented here allow us calculate stress-strain state of the shells under static and dynamic action of mechanical and thermal load.


## 6. Kirchhoff-Love’s Shell Equations

In the classical Kirchhoff-Love's theory of shells in addition to the assumptions of  Timoshenko's theory it is assumed thatεα3=0 and that the angles of rotation of the normal-to-middle surface vector become dependent; they are given by the equations
(55)uα1=-1Aα∂u30∂xα+kαuα0,orγα=-1Aα∂u3∂xα+kαuα.Substituting (55) with the kinematic equations for Timoshenko's shell theory we obtain kinematic equations for Kirchhoff-Love's shell theory in the form
(56)e11=1A1∂u1∂x1+1A1A2∂A1∂x2u2+k1u3,e22=1A2∂u2∂x2+1A1A2∂A2∂x1u1+k2u3,e12=1A2(∂u1∂x2-1A1∂A2∂x1u2)+1A1(∂u2∂x1-1A2∂A1∂x2u1),κ11=1A1∂γ1∂x1-1A1A2∂A1∂x2(1A2∂u3∂x2+k2u2),κ22=1A2∂γ2∂x2-1A1A2∂A2∂x1(1A1∂u3∂x1-k1u1),κ12=1A1A2∂A1∂x2(1A1∂u3∂x1-k1u1)-1A1∂γ2∂x1(1A2∂u3∂x2-k2u2)+k1ω2,κ21=1A1A2∂A2∂x1(1A2∂u3∂x2-k2u2)-1A2∂∂x2(1A1∂u3∂x1-k1u1)+k2ω1,ω1=1A1∂u2∂x1-1A1A2∂A1∂x2u1,ω2=1A2∂u1∂x2-1A1A2∂A2∂x1u2.
From two last equations of motion for Timoshenko's shell theory (50) we can find
(57)n13=1A1A2[∂(A2m11)∂x1+∂(A1m21)∂x2+m12∂A1∂x2-m22∂A2∂x1],n23=1A1A2[∂(A2m12)∂x1+∂(A1m22)∂x2+m21∂A2∂x1-m11∂A1∂x2].
Substituting them with other equations of motion (50) we obtain
(58)∂(A2n11)∂x1+∂(A1n12)∂x2+n12∂A1∂x2-n22∂A2∂x1+k1[∂(A2m11)∂x1+∂(A1m21)∂x2+m12∂A1∂x2-m22∂A2∂x1]+A1A2f1k=ρA1A2u¨1,∂(A2n12)∂x1+∂(A1n22)∂x2+n21∂A2∂x1-n11∂A2∂x1+k2[∂(A2m12)∂x1+∂(A1m22)∂x2+m21∂A2∂x1-m11∂A1∂x2]+A1A2f2k=ρA1A2u¨2,∂∂x1{1A1[∂(A2m11)∂x1+∂(A1m21)∂x2+m12∂A1∂x2-m22∂A2∂x1]}+∂∂x2{1A2[∂(A2m12)∂x1+∂(A1m22)∂x2+m21∂A2∂x1-m11∂A1∂x2∂(A2m12)∂x1]}-n11A1A2k1-n22A1A2k2+A1A2f3k=ρA1A2u¨3.In the same way substituting kinematic relations (56) with generalized Hooke’s law (51) and considering the result of the equations of motion (58) we obtain the following system of the differential equations in the form of displacements for Kirchhoff-Love's shell theory:
(59)Lijuj+∑k=01Likθk+A1A2bi=ρA1A2u¨i.Differential operators that appear in (59) for shells of arbitrary geometry have more complicated form; therefore they were not presented here.The equations of heat conductivity in Kirchhoff-Love's theory of shells have the same form as in  Vekua’s shells theory, that is, defined by (42).Components of the stress tensor can be calculated in the same way as for Timoshenko's shell theory using (54).


## 7. Comparative Study and Applications

Developed here is high order shell theory that gives us the full system of the equations for studying thermodynamical state of the thin-walled structures with high accuracy. We can keep in the polynomial expansion (20) as many terms as it is necessary for approximation of the stress-strain state with necessary accuracy. The only problem that may occur is that, on one hand more members one keeps, the more accurate results he has on the other hand the more members one keeps, the more complicated the system of equations he has to solve. Therefore general suggestion is that one has to keep as many members as it is necessary for getting results with necessary accuracy, but not more. We consider here in more detail first order theory which takes into account two members in the expansion (20) that theory is usually referred to as Vekua’s shell theory. Let us compare Vekua’s shell theory with classical Timoshenko’s and Kirchhoff-Love’s shell theories.Comparison of Vekua’s, Timoshenko’s, and Kirchhoff-Love’s shell theories has been done in Table1.Table 1
Vekua
σ
11
0
σ
12
0
σ
13
0
σ
22
0
σ
23
0
σ
33
0
σ
11
1
σ
12
1
σ
13
1
σ
22
1
σ
23
1
σ
33
1
Timoshenko
n
11
n
12
n
13
n
22
n
23
m
11
m
12
m
22
Kirchhoff-Love
n
11
n
12
n
13
n
22
n
23
m
11
m
12
m
22
Vekua
ε
11
0
ε
12
0
ε
13
0
ε
22
0
ε
23
0
ε
33
0
ε
11
1
ε
12
1
ε
13
1
ε
22
1
ε
23
1
ε
33
1
Timoshenko
e
11
e
12
e
13
e
22
e
23
κ
11
κ
12
κ
22
Kirchhoff-Love
e
11
e
12
e
22
κ
11
κ
12
κ
22
Vekua
u
1
0
u
2
0
u
3
0
u
1
1
u
2
1
u
3
1
Timoshenko
u
1
u
2
u
3
γ
1
γ
2
Kirchhoff-Love
u
1
u
2
u
3From Table1 it follows that Vekua’s shell theory considers all components of the stress-strain state in linear approximation. Classical theories are based on physical assumptions regarding stress and strain distribution. For example, according to static hypothesis σ33=0 and according to kinematic hypothesis ε33=0,  and therefore components σ330,σ331, and ε330,ε331 have no analogy in Timoshenko’s and Kirchhoff-Love’s shell theories. But on the other hand in classical theories ε33 is defined from the Hooke’s law using (52). Also in Kirchhoff-Love’s shell theory εα3=0 and in accordance with Hooke’s law σα3=0, and therefore nα3=0. But in fact  σα3 and nα3 are defined from the equations of equilibrium. Unfortunately classical theories contain some logical contradictions; nevertheless they are very popular and are frequently used in engineering applications.Systems of differential equations in displacements for Vekua’s (41), Timoshenko’s (53), and Kirchhoff-Love’s (59) theories for the case of arbitrary geometry shells are very complicated because of the structure of the differential operator presented in the Appendix Section. In order to simplify analysis of the structure of those equations, let us consider how they look for plates and cylindrical shells.


### 7.1. Equations in the Form of Displacements for Plates

All equations that specify thermodynamical state of the plates can be obtained from the general equations. In this case one has to substituteA1=A2=1 and k1=k2=0 and consider all the equations in Cartesian system of coordinates in order to obtain corresponding equations for the plates theory. We present in the following only differential equations in displacements for theories considered here.For Vekua’s theory differential equations in displacements have the form(60)μΔu10+(λ+μ)∂∂x1(∂u10∂x1+∂u20∂x2)+λh∂u31∂x1+βT∂θ0∂x1+f10=ρu¨10,μΔu20+(λ+μ)∂∂x2(∂u10∂x1+∂u20∂x2)+λh∂u31∂x2+βT∂θ0∂x2+f20=ρu¨20,μΔu30+μh(∂u11∂x1+∂u21∂x2)+f30=ρu¨30,μΔu11+(λ+μ)∂∂x1(∂u11∂x1+∂u21∂x2)-3μh(∂u30∂x1+1hu11)+βT(∂θ0∂x1+∂θ1∂x1)+f11=ρu¨11,μΔu21+(λ+μ)∂∂x2(∂u11∂x1+∂u21∂x2)-3μh(∂u30∂x2+1hu21)+βT(∂θ0∂x2+∂θ1∂x2)+f21=ρu¨21,μΔu31-3λh(∂u10∂x1+∂u20∂x2)+3(λ+2μ)h2u31-3βThθ0+f31=ρu¨31.For Timoshenko’s theory differential equations in displacements have the form(61)μΔu1+(λ+μ)∂∂x1(∂u1∂x1+∂u2∂x2)+βT∂θ0∂x1+f10=ρu¨10,μΔu2+(λ+μ)∂∂x2(∂u1∂x1+∂u2∂x2)+βT∂θ0∂x2+f20=ρu¨20,μΔu3+μ(∂γ1∂x1+∂γ2∂x2)+f3=ρu¨3,μΔγ1+(λ+μ)∂∂x1(∂γ1∂x1+∂γ2∂x2)-3μh(∂u3∂x1+γ1)+βT(∂θ0∂x1+∂θ1∂x1)+f11=ργ¨1,μΔγ2+(λ+μ)∂∂x2(∂γ1∂x1+∂γ2∂x2)-3μh(∂u3∂x2+γ2)+βT(∂θ0∂x2+∂θ1∂x2)+f21=ργ¨2.For Kirchhoff theory the differential equations in displacements have the form(62)μΔu1+(λ+μ)∂∂x1(∂u1∂x1+∂u2∂x2)+βT∂θ0∂x1+f1=ρu¨10,μΔu2+(λ+μ)∂∂x2(∂u1∂x1+∂u2∂x2)+βT∂θ0∂x2+f2=ρu¨20,μΔΔu3+βTΔθ1+f3=ρu¨3.System of differential equations for Vekua’s theory (60) is coupled, and all equations have to be solved together. In Timoshenko’s and Kirchhoff’s theories the first two equations are independent and can be solved separately. Also in Timoshenko’s theory equations for the plate deflection u3 and angles of rotation γα are coupled (61) whereas in Kirchhoff’s theory we have only one equation for the plate deflection u3 of the from (62).System of differential equations of the heat conductivity is the same for all plate theories considered here and has the form (42), where differential operators have simpler form in Cartesian system of coordinates.


### 7.2. Equations in the Form of Displacements for Cylindrical Shells

All equations that specify thermodynamical state of the cylindrical shell can be obtained from general equations presented here. In this case one has to introduce cylindrical coordinates in the following way:x1=rξ,x2=rϑ, and substitute A1=A2=r,k1=0,k2=r-1. After that all corresponding equations for the cylindrical shell theory can be easily obtained. Differential equations in displacements for cylindrical shells have the same structure as in general case but differential operators are much simpler. We present them here.For Vekua’s theory differential operators have the form(63)L1100=μΔ+(λ+μ)∂2∂ξ2,L1200=(λ+μ)∂2∂ξ∂ϑ,L1300=λ∂∂ξ,L1101=0,L1201=0,L1301=λrh∂∂ξ,L2100=(λ+μ)∂2∂ξ∂ϑ,L2200=μΔ+(λ+μ)∂2∂ϑ2-μ,L2300=(λ+2μ)∂∂ϑ+μ∂∂ϑ,L2101=0,L2201=μrh,L2301=λrh∂∂ϑ,L3100=-λ∂∂ξ,L3200=-μ∂∂ϑ-(λ+2μ)∂∂ϑ,L3300=-μΔ-(λ+2μ),L3101=-μrh∂∂ξ,L3201=-μrh∂∂ϑ,L3301=-λrh,L1110=0,L1210=0,L1310=-μ3rh∂∂ξ,L1111=L1100-μ3r2h2,L1211=L1200,L1311=L1300,L2110=0,L2210=μ3rh,L2310=-μ3rh∂∂ϑ,L2111=L1200,L2211=L2200-μ3r2h2,L2311=L2300,L3110=-λ3rh∂∂ξ,L3210=-λrh∂∂ϑ,L3310=-λ3rh,L3111=L3100,L3211=L3200,L3311=L3300-(λ+2μ)3r2h2.For Timoshenko’s theory differential operators have the form(64)L1100=Dn(∂2∂ξ2+1-υ2∂2∂ϑ2),L1200=L2100=Dn1+υ2∂2∂ξ∂ϑ,L1300=L3100=Dnυ∂∂ξ,L1101=L1110=L1201=L1110=0,L2200=Dn(1-υ2∂2∂ξ2+∂2∂ϑ2-1-υ2),L2101=L2110=0,L2300=-L3200=Dn(∂∂ξ+1-υ2∂∂ϑ),L2201=L2210=Ehr1+υ,L3101=-L1310=Ehr1+υ∂∂ξ,L3201=-L2310=Ehr1+υ∂∂ϑ,L3300=Dnr2(1-υ2Δ-1r2),L1211=L2111=Dm1+υ2∂2∂ξ∂ϑ,L1111=Dm(∂2∂ξ2+1-υ2∂2∂ϑ2),L2211=Dm(1-υ2∂2∂ξ2+∂2∂ϑ2).
Here Dn=2Eh/(1-υ2) is a stiffness that corresponds to in-plane deformation, and Dm=2Eh3/ (3(1-υ2)) is a stiffness that corresponds to bending deformation.For Kirchhoff-Love's theory differential operators have the form(65)L11=Dn(∂2∂ξ2+1-υ2∂2∂ϑ2),L12=L21=Dn1+υ2∂2∂ξ∂ϑ,L13=-L31=Dnυ∂∂ξ,L22=Dn(1-υ2∂2∂ξ2+∂2∂ϑ2-1-υ2)+Dm1r2(2(1-υ)∂2∂ξ2+∂2∂ϑ2),L23=-L32=Dn∂∂ϑ-Dm1r2((2-υ)∂3∂ξ2∂ϑ+∂3∂ξ3),L33=-Dn-DmΔΔ.System of differential equations of the heat conductivity is the same for all cylindrical shell theories considered here and has the form (42), where differential operators have simpler form in cylindrical system of coordinates.


## 7.1. Equations in the Form of Displacements for Plates

All equations that specify thermodynamical state of the plates can be obtained from the general equations. In this case one has to substituteA1=A2=1 and k1=k2=0 and consider all the equations in Cartesian system of coordinates in order to obtain corresponding equations for the plates theory. We present in the following only differential equations in displacements for theories considered here.For Vekua’s theory differential equations in displacements have the form(60)μΔu10+(λ+μ)∂∂x1(∂u10∂x1+∂u20∂x2)+λh∂u31∂x1+βT∂θ0∂x1+f10=ρu¨10,μΔu20+(λ+μ)∂∂x2(∂u10∂x1+∂u20∂x2)+λh∂u31∂x2+βT∂θ0∂x2+f20=ρu¨20,μΔu30+μh(∂u11∂x1+∂u21∂x2)+f30=ρu¨30,μΔu11+(λ+μ)∂∂x1(∂u11∂x1+∂u21∂x2)-3μh(∂u30∂x1+1hu11)+βT(∂θ0∂x1+∂θ1∂x1)+f11=ρu¨11,μΔu21+(λ+μ)∂∂x2(∂u11∂x1+∂u21∂x2)-3μh(∂u30∂x2+1hu21)+βT(∂θ0∂x2+∂θ1∂x2)+f21=ρu¨21,μΔu31-3λh(∂u10∂x1+∂u20∂x2)+3(λ+2μ)h2u31-3βThθ0+f31=ρu¨31.For Timoshenko’s theory differential equations in displacements have the form(61)μΔu1+(λ+μ)∂∂x1(∂u1∂x1+∂u2∂x2)+βT∂θ0∂x1+f10=ρu¨10,μΔu2+(λ+μ)∂∂x2(∂u1∂x1+∂u2∂x2)+βT∂θ0∂x2+f20=ρu¨20,μΔu3+μ(∂γ1∂x1+∂γ2∂x2)+f3=ρu¨3,μΔγ1+(λ+μ)∂∂x1(∂γ1∂x1+∂γ2∂x2)-3μh(∂u3∂x1+γ1)+βT(∂θ0∂x1+∂θ1∂x1)+f11=ργ¨1,μΔγ2+(λ+μ)∂∂x2(∂γ1∂x1+∂γ2∂x2)-3μh(∂u3∂x2+γ2)+βT(∂θ0∂x2+∂θ1∂x2)+f21=ργ¨2.For Kirchhoff theory the differential equations in displacements have the form(62)μΔu1+(λ+μ)∂∂x1(∂u1∂x1+∂u2∂x2)+βT∂θ0∂x1+f1=ρu¨10,μΔu2+(λ+μ)∂∂x2(∂u1∂x1+∂u2∂x2)+βT∂θ0∂x2+f2=ρu¨20,μΔΔu3+βTΔθ1+f3=ρu¨3.System of differential equations for Vekua’s theory (60) is coupled, and all equations have to be solved together. In Timoshenko’s and Kirchhoff’s theories the first two equations are independent and can be solved separately. Also in Timoshenko’s theory equations for the plate deflection u3 and angles of rotation γα are coupled (61) whereas in Kirchhoff’s theory we have only one equation for the plate deflection u3 of the from (62).System of differential equations of the heat conductivity is the same for all plate theories considered here and has the form (42), where differential operators have simpler form in Cartesian system of coordinates.


## 7.2. Equations in the Form of Displacements for Cylindrical Shells

All equations that specify thermodynamical state of the cylindrical shell can be obtained from general equations presented here. In this case one has to introduce cylindrical coordinates in the following way:x1=rξ,x2=rϑ, and substitute A1=A2=r,k1=0,k2=r-1. After that all corresponding equations for the cylindrical shell theory can be easily obtained. Differential equations in displacements for cylindrical shells have the same structure as in general case but differential operators are much simpler. We present them here.For Vekua’s theory differential operators have the form(63)L1100=μΔ+(λ+μ)∂2∂ξ2,L1200=(λ+μ)∂2∂ξ∂ϑ,L1300=λ∂∂ξ,L1101=0,L1201=0,L1301=λrh∂∂ξ,L2100=(λ+μ)∂2∂ξ∂ϑ,L2200=μΔ+(λ+μ)∂2∂ϑ2-μ,L2300=(λ+2μ)∂∂ϑ+μ∂∂ϑ,L2101=0,L2201=μrh,L2301=λrh∂∂ϑ,L3100=-λ∂∂ξ,L3200=-μ∂∂ϑ-(λ+2μ)∂∂ϑ,L3300=-μΔ-(λ+2μ),L3101=-μrh∂∂ξ,L3201=-μrh∂∂ϑ,L3301=-λrh,L1110=0,L1210=0,L1310=-μ3rh∂∂ξ,L1111=L1100-μ3r2h2,L1211=L1200,L1311=L1300,L2110=0,L2210=μ3rh,L2310=-μ3rh∂∂ϑ,L2111=L1200,L2211=L2200-μ3r2h2,L2311=L2300,L3110=-λ3rh∂∂ξ,L3210=-λrh∂∂ϑ,L3310=-λ3rh,L3111=L3100,L3211=L3200,L3311=L3300-(λ+2μ)3r2h2.For Timoshenko’s theory differential operators have the form(64)L1100=Dn(∂2∂ξ2+1-υ2∂2∂ϑ2),L1200=L2100=Dn1+υ2∂2∂ξ∂ϑ,L1300=L3100=Dnυ∂∂ξ,L1101=L1110=L1201=L1110=0,L2200=Dn(1-υ2∂2∂ξ2+∂2∂ϑ2-1-υ2),L2101=L2110=0,L2300=-L3200=Dn(∂∂ξ+1-υ2∂∂ϑ),L2201=L2210=Ehr1+υ,L3101=-L1310=Ehr1+υ∂∂ξ,L3201=-L2310=Ehr1+υ∂∂ϑ,L3300=Dnr2(1-υ2Δ-1r2),L1211=L2111=Dm1+υ2∂2∂ξ∂ϑ,L1111=Dm(∂2∂ξ2+1-υ2∂2∂ϑ2),L2211=Dm(1-υ2∂2∂ξ2+∂2∂ϑ2).
Here Dn=2Eh/(1-υ2) is a stiffness that corresponds to in-plane deformation, and Dm=2Eh3/ (3(1-υ2)) is a stiffness that corresponds to bending deformation.For Kirchhoff-Love's theory differential operators have the form(65)L11=Dn(∂2∂ξ2+1-υ2∂2∂ϑ2),L12=L21=Dn1+υ2∂2∂ξ∂ϑ,L13=-L31=Dnυ∂∂ξ,L22=Dn(1-υ2∂2∂ξ2+∂2∂ϑ2-1-υ2)+Dm1r2(2(1-υ)∂2∂ξ2+∂2∂ϑ2),L23=-L32=Dn∂∂ϑ-Dm1r2((2-υ)∂3∂ξ2∂ϑ+∂3∂ξ3),L33=-Dn-DmΔΔ.System of differential equations of the heat conductivity is the same for all cylindrical shell theories considered here and has the form (42), where differential operators have simpler form in cylindrical system of coordinates.


## 8. Conclusions

In this paper a high order theory for homogeneous thermoelastic shells has been developed. The proposed approach is based on expansion of the coupled equations of thermoelasticity and heat conductivity into Fourier series in terms of Legendre polynomials. Starting from the equations of coupled thermoelasticity and heat conductivity, stress and strain tensors, vectors of displacements, traction and body forces, temperature, and vector of thermal flow have been expanded into Fourier series in terms of Legendre polynomials in a thickness coordinate. Thereby all equations of thermoelasticity including generalized Hooke’s law and equations of heat conductivity have been transformed to corresponding equations for Fourier coefficients of Legendre’s polynomial expansion. The system of differential equations in terms of displacements including initial and boundary conditions for Fourier coefficients has been obtained. Special attention has been paid to the case of the first approximation shells theory. All equations of thermoelasticity and heat conductivity for Vekua’s, Timoshenko’s, and Kirchhoff-Love’s shell theories have been obtained. Differential operator for shells of arbitrary geometry, cylindrical shells, and plates has been obtained and presented in the explicit form. Comparison of Vekua’s, Timoshenko’s, and Kirchhoff-Love’s shell theories has been done, and corresponding equations have been analyzed. Obtained equations can be used for thermomechanical analysis of the shells of any specific geometry and also for numerical calculations.



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*Source: 590480-2013-03-07.xml*