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- 1. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012 Natural Frequencies of Magnetoelastic Longitudinal Wave Propagation in an Orthotropic Circular Cylinder 1, 2 * 3 Abo-el-nour N. Abd-alla and Aishah Raizah1 Department of Mathematics, Faculty of Science, Jazan University, Jazan, Saudi Arabia2 Department of Mathematics, Faculty of Science, Sohag University, Sohag, Egypt.3 Department of Mathematics, Science College, King Khalid University, Abha, Saudi Arabia* E-mail address: aboelnourabdalla@yahoo.comAbstractIn this paper, we study the longitudinal wave propagation in a perfectly conducting elastic circular cylinder in the presenceof an axial initial magnetic field. The elastic cylinder is assumed to be made of an orthotropic material. The problem isrepresented by the equations of elasticity taking into account of the effect of the magnetic field as given by Maxwellsequations in the quasi-static approximation. The stress free conditions on the inner and outer surfaces of the hollowcircular cylinder are used to form a frequency equation in terms of the wavelength, the cylinder radii and the materialconstants. Numerical calculations are obtained and the results are represented graphically. It is observed that the longitudinalelastic waves in a solid body propagating under the influence of a superimposed magnetic field can be different significantlyfrom that of those propagating in the absence of a magnetic field. Also, elastic waves may convey information onelectromagnetic properties of the material: for example through a precise measurement of the surface current induced by thepresence of the magnetic field. Finally, some of the earlier results are deduced as particular cases.Keywords: Natural frequencies, Magnetoelasticity, Longitudinal wave, Orthotropic materials,1. IntroductionLongitudinal waves are waves that have vibrations along or parallel to their direction of travel; that is, waves in whichthe motion of the medium is in the same direction as the motion of the wave. The study of wave propagation over acontinuous media is of practical importance in the field of engineering, medicine, optics science, seismology,acoustics and in space science.With the advancement of space research, it has become necessary to obtain a deep insight in the behavior of materials,especially of the anisotropic ones that are so frequently used in the missiles and other allied systems. Without takingthe consideration of the effect of the magnetic field, the analysis of longitudinal wave propagation in anisotropic andhomogeneous circular cylindrical shell, according to the theory of elasticity, have been done by many authors: [1, 2, 3,4, 5]. Moreover, the propagation of harmonic waves, in circular cylinders which are made of isotropic or anisotropicmaterials, have been investigated and evaluated numerically, on the basis of the theory of elasticity, by Mirsky [6],Tsai [7] and White and Tongtaow [8].Among many important problems which are considered in such studies, the problems of elastic wave propagation inthe presence of a steady magnetic field have investigated when the material was isotropic homogeneous by Andreou etal. [9], Das et al. [10], Gourakishwar [11], Paria [12], Suhubi [13]. Some of the analogous results on magnetoelastic 7
- 2. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012waves propagation problems, but in an anisotropic medium, were obtained by Abd-alla [14, 15], Datta [16]. Generaldetails and many references on these subjects may be found in monographs published by: Eringen et al. [17-18], Auld[19], Moon [20] and Nowacki [21].Recently, the interaction of electromagnetic fields with the motion of a deformable solid is being receiving greaterattention by many investigators. Therefore, many researchers investigated the effect of the magnetic field on the wavepropagation in anisotropic cylindrical materials such as: Barakati and Zhupanska [22] studied the effects of pulsedelectromagnetic fields on the dynamic mechanical response of electrically conductive anisotropic plates. Dinzart andSabar [23] presented numerical investigations into magneto-electro-elastic moduli responsible for the magneto-electric coupling as functions of the volume reaction and characteristics of the coated inclusions. Akbarovet al. [24]studied torsional wave dispersion in a three-layered (sandwich) hollow cylinder with finite initial strains.Chattopadhyay et al. [25] studied the propagation of horizontally polarized shear waves in an internal magnetoelasticmonoclinic stratum with irregularity in lower interface. Tang and Xu [26] employed the method of eigenfunctionexpansion to solve the problems of transient torsional vibration responses of finite, semi-infinite and infinite hollowcylinders. Acharya et al. [27] investigated the effect of the transverse isotropy and magnetic field on the interfacewaves in a conducting medium subject to the initial state of stress of the form of hydrostatic tension or compression.Petrov et al. [28] focused on the nature of ferromagnetic resonance (FMR) under the influence of acoustic oscillationswith the same frequency as FMR. Mol’chenko et al. [29] constructed a two-dimensional nonlinear magnetoelasticmodel of a current-carrying orthotropic shell of revolution taking into account of finite orthotropic conductivity,permeability and permittivity. Abd-Alla and Abo-Dahab [30] studied the influence of the viscosity on reflection andrefraction of plane shear elastic waves in two magnetized semi-infinite media. Selim [31] showed the effect ofdamping on the propagation of torsional waves in an initially stressed, dissipative, incompressible cylinder of infinitelength. Dai and Wang [32] illustrated an analytical method to solve magneto-elastic wave propagation andperturbation of the magnetic field vector in an orthotropic laminated hollow cylinder with arbitrary thickness. Liu andChang [33] investigated the interactive behaviors among transverse magnetic fields, axial loads and external force ofa magneto-elastic beam with general boundary conditions. In this study an attempt has been made to investigate the longitudinal wave propagation in an orthotropic circularcylinder permeated by a magnetic field. The frequency equations have been derived in the form of a determinantinvolving Bessel functions and its roots give the values of the characteristic circular frequency parameters of the firstthree modes for various geometries. These roots, which correspond to various mode, have been verified numericallyand represented graphically in different values for the magnetic field. Finally, some of the earlier results are deducedas particular cases. 2. Basic EquationsThe equations of motion for a perfect conducting elastic solid in uniform magnetic field are [10]: τ ji , j + f i = ρui && i,j=1,2,3 (1)where τ ij is the mechanical stress tensor, ρ is the mass density of the material, f i is Lorentz force and given asfollows: r µ r r r f = o [∇ × h ] × H 0 (2) 4π 8
- 3. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012where ( ) r r r r h = ∇× u × Ho (3) r H o = (0,0, H o ) (4) rand H o is the intensity of the uniform axial magnetic field , h small perturbation of the magnetic field, µo is the rmagnetic permeability in the medium. From (3) and (4) h may be written as: r ∂u r ∂u u r h = Ho er − H o + e z (5) ∂z ∂r r Using (4) and (5) in (2), Lorentz force becomes: r ∂ 2 u 1 ∂u u ∂ 2 u r f = ρα 2 2 + − + er (6) ∂r r ∂r r 2 ∂z 2 µo H o 2where α2 = 4πρMaxwells equations in this study may be written as (in Gaussian units): v r r 4π r r r 1 ∂B r v r v ∇× H = J, ∇× E = − , ∇ ⋅ B = 0, ∇ ⋅ D = ρe (7) c c ∂t r v v vwhere H , B, E , J denote, respectively, the magnetic field intensity, magnetic induction, electric field intensity and currentdensity vectors, c is the velocity of light in vacuum, and the electric field intensity is given as the form µ o H o ∂u Eθ = [ ] (8) c ∂tElectromagnetic equations in vacuum are: r 2 1 ∂ 2 v* v * 1 ∂ v * v* ( ) ( ) ( ) v v ∇ − 2 2 h , E = 0, curl h * , E * = E ,− h (9) c ∂t c ∂twhere ∂2 1 ∂ 1 ∂2 ∇ = 2+ 2 + ∂r r ∂r r 2 ∂θ 2The strain components are given in terms of the displacements by: ∂u u ∂w err = , eθθ = , ezz = , ∂r r ∂z 9
- 4. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012 1 ∂u ∂w (10) erz = [ + ], erθ = 0 , eθz = 0 . 2 ∂z ∂rwhere eij denote the strain components.For an orthotropic elastic body, the Cauchy stress components are given in terms of independent elastic constants c ij asfollows ∂u u ∂w ∂u u ∂w τ rr = c11 + c12 + c13 , τ θθ = c12 + c11 + c13 , ∂r r ∂z ∂r r ∂z ∂u u ∂w ∂w ∂u τ zz = c13 + c13 + c33 , τ rz = c44 ( + ), ∂r r ∂z ∂r ∂z (11) τ zθ = 0, τ rθ = 0 .Substituting (6) and (11) into (1), one may get the equations of motion in terms of the displacements components as: ∂ 2 u u 1 ∂u ∂2w ∂ 2u ∂ 2 w c11 2 − 2 + + c13 + c 44 2 + ∂r r r ∂r ∂r∂z ∂z ∂r∂z (12) ∂ 2 u 1 ∂u u ∂ 2 u ∂ 2u + ρα 2 + 2 − 2 + 2=ρ 2 ∂r r ∂r r ∂z ∂t u 1 ∂u ∂2w ∂ 2 w 1 ∂w [c44 + c13 ] ∂ ∂2w 2 + + c33 2 + c 44 2 + =ρ 2 (13) ∂r∂z r ∂z ∂z ∂r r ∂r ∂t3. Formulation of the ProblemLongitudinal wave propagation in a circular cylinder of tetragonal elastic material of inner and outer radii, a and b,subjected to an axial magnetic field is considered. The cylinder is treated as a perfect conductor and the regions inside andoutside the elastic material are assumed to be vacuum. We assume that waves are characterized by the displacement components in the radial and axial directions only. Thedisplacement field, in this case, in cylindrical coordinates (r, θ , z), is given by u = u(r , z, t ), v = 0, w = w(r , z, t ), (14)where u , v, w are the displacement components in the radial, circumferential, and axial directions, respectively, and allother quantities involved are functions of r, z and t only, where t denotes the time.4. Solution of the Problem4.1. Harmonic solutions:We now consider the propagation of an infinite strain of sinusoidal waves along a hollow circular cylinder of infiniteextent such that the displacement at each point is a sample harmonic function of z and t . Therefore, we shall seek thesolution of the equations of motion and follow the same procedure as in Mirsky [6]: dφ u (r , z, t ) = cos(λt + qz ), w(r , z, t ) = ηφ sin (λt + qz ) (15) dr 10
- 5. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012 2πwhere φ = φ (r ) , q = is the wave number, l is the wavelength, λ is the angular frequency and η is an larbitrary constant to be determined later in the analysis. Putting Eq. (15) in (13) and (14), one obtains: ( ) d 2φ 1 dφ ρλ2 − c 44 + ρα 2 q 2 + ηq(c 44 + c13 ) 2 + dr + φ = 0 (16) r dr c11 + ρα 2 ( d 2φ 1 dφ η ρλ2 − q 2 c33 ) 2 + dr + φ = 0 r dr ηc44 − q(c 44 + c13 ) (17)Eq. (16) is consistent with (17) provided that η is chosen to satisfy the equations η (ρλ2 − q 2 c33 ) ρλ2 − (c 44 + ρα 2 )q 2 + ηq(c 44 + c13 ) = = P2 (18) ηc 44 − q(c 44 + c13 ) c11 + ρα 2Eliminating η from (18), we find that p 2 satisfies the equation: A( p 2 ) 2 + Bp 2 + C = 0 (19)where ( A = c 44 c11 + ρα 2 , ) ( ) ( ( B = −[ ρλ2 c11 + ρα 2 + c 44 + q 2 c13 + c 44 2c13 − ρα 2 − c33 c11 − ρα 2 c33 2 ) ) (20) ( )( C = ρλ2 − q 2 c33 ρλ2 − ρα 2 q 2 − c 44 q 2 ) If p12 and p 2 are the roots of this equation, the corresponding functions φ1 = φ1 (r ), φ2 = φ 2 (r ) satisfy the 2equations: d 2φ1 1 dφ1 2 d 2φ 2 1 dφ 2 2 [ + ] + p1 φ1 = 0, [ + ] + p 2 φ 2 = 0, (21) dr 2 r dr dr 2 r drwhere −B−D −B+D P12 = , P22 = ; D = B 2 − 4 AC 2A 2AThe general solutions of Eqs. (21) are φ1 (r ) = A1Z 0 ( P1r ) + B1W0 ( P1r ), φ 2 (r ) = A2 Z 0 ( P2 r ) + B2W0 ( P2 r ), (22)where A1 , B1 , A2 and B2 are constants of integration and for brevity Z denote the Bessel function J or I and W denotethe Bessel function Y or K, according to the signs of p12 and p 2 . 2 The displacement field may now be written as 11
- 6. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012 dφ1 dφ 2 u =[ + ] cos(λt + qz ), w = [η1φ1 + η 2φ 2 ] sin(λt + qz ) (23) dr drwhere η1 = (c44 + ρα 2 )q 2 − ρλ2 + P12 (c11 + ρα 2 ), η2 = q (c 44 + c13 )P2 2 (24) q(c44 + c13 ) c44 P2 − ρλ2 + q 2 c33 24.2. Solution of Electric field intensity in vacuum * The general solution of Eθ from (10) 4 take the form A3 Z 0 (kr ) sin(λt + qz ), r ≤ a E* = (25) B3W0 (kr ) sin(λt + qz ), r ≥ bwhere k = (λ2 / c 2 ) − q 2 , A3 and B3 are arbitrary constants and for brevity W denotes the Bessel function Y or 2K, according to the signs of k .4.3. Boundary conditions: For free motion, the boundary conditions are required for the total stress to be vanished and the continuity of the electricfield on the surfaces r = a, b, i.e. τ rr + M rr − M rr = 0 * τ rz + M rz − M rz = 0 on r = a, b * (26) E=E * where τ rr ,τ rz are the components of the mechanical stresses, M rr , M rz are the components of Maxwells stresses in * *the medium and M rr , M rz are Maxwells stresses in vacuum. Eliminating A1 , A2 , B1 , B2 , A3 , B3 after applying theboundary conditions (26), we get the determinant must be vanished leading to the following frequency equation(dispersion relation) as: ∆ = X ij = 0, i, j = 1,2,....6 (27)where 12
- 7. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012 Pδ X 11 = (c11 + ρα 2 ) P 2 Z 2 ( P a ) − (c11 + c12 + 2 ρα 2 ) 1 Z1 ( P a ) + qc13η1Z 0 ( P a ), 1 1 1 1 a P X 12 = (c11 + ρα 2 ) P 2W2 ( P a ) − (c11 + c12 + 2 ρα 2 ) 1 W1 ( P a ) + qc13η1W0 ( P a), 1 1 1 1 a Pδ X 13 = (c11 + ρα 2 ) P2 Z 2 ( P2 a ) − (c11 + c12 + 2 ρα 2 ) 2 Z1 ( P2 a) + qc13η1Z 0 ( P2 a ), 2 a P X 14 = (c11 + ρα 2 ) P2 W2 ( P2 a) − (c11 + c12 + 2 ρα 2 ) 2 W1 ( P2 a) + qc13η1W0 ( P2 a), 2 a cH 0 1 X 15 = 4πλ a Z 0 (ka ) − δkZ1 (ka ), X 16 = 0, PδX 21 = (c11 + ρα 2 ) P 2 Z 2 ( P b) − (c11 + c12 + 2 ρα 2 ) 1 Z1 ( P b) + qc13η1Z 0 ( P b), 1 1 1 1 b PX 22 = (c11 + ρα 2 ) P 2W2 ( P b) − (c11 + c12 + 2 ρα 2 ) 1 W1 ( P1b) + qc13η1W0 ( P b), 1 1 1 b (28) PδX 23 = (c11 + ρα 2 ) P2 Z 2 ( P2 b) − (c11 + c12 + 2 ρα 2 ) 2 Z1 ( P2 b) + qc13η1Z 0 ( P2 b), 2 b P2X 24 = (c11 + ρα 2 ) P2 W2 ( P2 b) − (c11 + c12 + 2 ρα 2 ) W1 ( P2 b) + qc13η1W0 ( P2 b), 2 bX 25 = 0, H 0c 1 X 26 = b W0 (kb) − kW1 (kb), 4πλ − c η + q(c 44 + ρα 2 ) − c η + q(c44 + ρα 2 ) X 31 = 44 1 δP1 Z 1 ( P1 a ), X 32 = 44 1 PW ( P a ), 2 1 1 1 − c 44η 2 + q (c 44 + ρα 2 ) − c44η 2 + q (c44 + ρα ) X 33 = δP2 Z1 ( P2 a ), X 34 = P2W1 ( P2 a ), qH 0c Z 0 (ka ) X 36 = 0,X 35 = , 4πλ − c44η 2 + q (c44 + ρα 2 ) − c η + q(c44 + ρα 2 ) − c η + q(c + ρα 2 ) X 41 = 44 1 δP Z ( P b), 2 1 1 1 X 42 = 44 1 44 P W1 ( P b), 1 1 − c44η 2 + q(c44 + ρα ) 2 − c44η 2 + q (c44 + ρα ) X 43 = δP2 Z1 ( P2 b), X 44 = P2W1 ( P2b), qH 0 c W0 (kb) X 46 = ,X 45 = 0, 4πλ − c44η 2 + q(c44 + ρα 2 ) 13
- 8. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012 λH 0 λH 0δ X 52 = P W1 ( P a ), 1 1X 51 = P Z1 ( P a ), 1 1 c c λH 0 λH 0δ X 54 = P2W1 ( P2 a ),X 53 = P2 Z1 ( P2 a ), c cX 55 = Z 0 (ka), X 56 = 0, λH 0 λ H 0δ X 62 = P W1 ( P b), 1 1X 61 = P Z1 ( P b), 1 1 c c λH 0 λH 0 δ X 64 = P2W1 ( P2b),X 63 = P2 Z1 ( P2 b), c cX 65 = 0, X 66 = W0 (kb).where δ =1 at Z = J and δ = −1 at Z = I .5. Radial and Axial VibrationsAs the wave number q → 0 (i.e., for infinite wavelength), the following simplifications have been made by using theresult of [6]: q 2 = 0, ρλ2 P → 1 c11 + ρα 2 λ2 ρλ2 k→ , P2 → , c2 c44 (c − c + ρα 2 )ρλ2 , qη1 → 11 44 qη 2 → q 2 (c44 + c13 ) , c44 (c44 + c13 ) c44 − c11 − ρα 2 q [− c 44η1 + q (c44 + ρα 2 ) ] → 0. [− c 44η 2 + q (c44 + ρα ) 2 ] → 0, [− c 44η 2 + q (c44 + ρα 2 )]and the characteristic equation (27) may be written as the product of two determinants ∆1 ⋅ ∆ 2 = 0 (29)where 14
- 9. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012 X 11 X 12 X 15 0 X 21 X 22 0 X 26 ∆1 = = 0, X 33 X 34 X 51 X 52 X 55 0 ∆2 = = 0. (30) X 43 X 44 X 61 X 62 0 X 66The elements X ij are given by (28) with q → 0 . The equation ∆1 = 0 represents a motion involving the radialdisplacement u only, corresponding to the radial vibrations [15]. ∆ 2 = 0 represents a motion involving the axialdisplacement w only, corresponding to the axial-shear vibrations [6] and [13].6. The Numerical CalculationsFor numerical calculations, we consider the following transformations: λ γ γ Ω= λi = , β= , c44 , b c γ= , λi ρ a 2π 2πb Ω1 = γΩ, h= , q= , m= . b l lThe calculations of the roots of the frequency equation (27), represent a major task and require a rather extensive effort fornumerical computation. Calculations have been carried out for the case of Titanium dioxide (Rutile TiO2 ), whichbelongs to the tetragonal system (crystal symmetry for it is 4/mmm). It has 6 elastic constants [19]. c11 = 26.6(1011 ) dyne / cm 2 c33 = 46.99(1011 ) dyne / cm 2 c12 = 17.33(1011 ) dyne / cm 2 c 44 = 12.39(1011 ) dyne / cm 2 c13 = 13.62(1011 ) dyne / cm 2 c 66 = 17.33(1011 ) dyne / cm 2Also, the density is ρ = 4.26 gm / cm 3 , the velocity of light is c = 3(1010 ) cm / sec and the permeability isµ o = 1 Gauss / Oersted c = 3(1010 ) cm / sec .7. Discussion and ConclusionThe dimensionless frequency spectrum Ω for the longitudinal vibrations, as a function of the ratio thickness h = ( a / b) ,for the value of non-dimensional wave number m = 1 , is calculated and given in form of graphs. The values of theeffective primary magnetic field H o are chosen as ( H o = 105 ,10 6 ,10 7 Oersted). The frequency equation is solvednumerically, and for this purpose a matrix determinant computation routine is used for different Ω and h along with a rootfinding method to refine steps close to its roots. For each pair ( Ω and h ), Eqs. (27) and (30) are solved by using "intervalhalving" iteration technique [34]. The results in these cases are presented in the Figures (1-9) to illustrate the effects of the 15
- 10. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012primary magnetic field on the longitudinal vibrations of an orthotropic circular cylinder.It is clear from Figure 1. The first mode of dimensionless frequency decreases as the ratio thickness h increases for( Ho = 105 ,10 6 Oersted). However, it increases monotonically as function of h for the value of primary magnetic fieldincreases ( H o = 10 7 Oersted). The same behavior is observed for the case of ( H o = 105 ,10 6 ,10 7 Oersted) and it isshown in Figures 2 and 3 for the second and third modes of dimensionless frequency . Also, in this case the effects of theprimary magnetic field when ( H o = 105 ,10 6 Oersted) are very small and the curves are almost identical. In Figure 4 acomparison between the first three modes of the frequency versus different values of h for H o = 10 7 is illustrated.Furthermore, our numerical calculations show that all the mode of the frequency is not sensitive to the primary magneticfield H o less than 10 5 Oersted. So, for the values of H o less than 10 5 , it can be neglected as their relative variationsbecome less than 10 3 .It is clarified that when m = 0 , the frequency equation (27) degenerates into two independent equations: (i) One ofthem is for uncoupled radial vibrations (which contains the radial displacement u only). (ii) The second shows axialshear vibrations (which contains the axial displacement w only). The first, second and third modes of the 6dimensionless frequency Ω as function of the h of radial vibrations for various values of H o = (1, 5, 10)10 arepresented in Figures 5, 6 and 7 respectively. Furthermore, in the same case, a comparison between the first threemodes of the frequency as a function of h when H o = 5 × 10 6 is shown in Figure 8. It is visible that in this caseall modes are increase when increasing the imposed magnetic field H o . Figure 9, represents the first three modes ofdimensionless frequency of axial shear vibrations against the variation of h when m=0. It was found that in thissecond special case, the frequency of axial shear vibrations is not affected with the values of the primary magneticfield H o . Finally, some existing results in the literature are considered as the special case of this study, for exampleRefs. [6, 7, 8, 10, 15, 16].References[1] Srinil, N. and Rega, G., (2008) "Nonlinear longitudinal/transversal modal interactions in highly extensible suspended cables", J. Sound and Vibration, 310, pp.230-242.[2] Honarvar, F., Enjilela, E., Sinclair, A.N. and Mirnezami, S. A., (2007) "Wave propagation in transversely isotropic cylinders", Int. J. solid and Structures, 44, pp.5236-5246.[3] Anderson, S.P., (2006) "Higher-order rod approximations for the propagation of longitudinal stress waves in elastic bars, J. Sound and Vibration", 290, pp.290-308.[4] Ting, T.C.T., (2006) "Longitudinal and transverse waves in anisotropic elastic materials", Acta Mechanica, 185, pp147-164. 16
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- 12. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012[27] Acharya D.P., Roy I. and Sengupta S., (2009) "Effect of magnetic field and initial stress on the propagation of interface waves in transversely isotropic perfectly conducting media", Acta Mech 202, pp.35–45.[28] Petrov V.M., Zibtsev V.V. and Srinivasan G., (2009) " Magnetoacoustic resonance in ferrite-ferroelectric nanopillars", Eur. Phys. J. B 71, pp.367–370.[29] Mol’chenko L.V., Loos I. I., and Indiaminov R. Sh., ( 2008) " Determining the stress state of flexible orthotropic shells of revolution in magnetic field", International Applied Mechanics, 44( 8), pp.882-891.[30] Abo-el-Nour N. Abd-Alla and S.M. Abo-Dahab, (2008) "The influence of the viscosity and the magnetic field on reflection and transmission of waves at interface between magneto-viscoelastic materials", Meccanica 43 pp.437–448.[31] Selim, M. M, (2007) "Torsional waves propagation in an initially stressed dissipative cylinder", Applied Mathematical Sciences, 1(29), pp.1419 – 1427.[32] Dai H.L., Wang X., (2006) "Magnetoelastodynamic stress and perturbation of magnetic field vector in an orthotropic laminated hollow cylinder", International Journal of Engineering Science 44 pp.365–378.[33] Liu M.F. and Chang T.P., (2005) "Vibration analysis of a magneto-elastic beam with general boundary conditions subjected to axial load and external force", Journal of Sound and Vibration, 288(1-2), pp. 399-411.[34] Rao S.S., (2001) "Applied numerical methods for engineers and scientists", Pearson Inc. U.K. Figure 1. The first mode of dimensionless frequency for longitudinal vibrations versus different values of h=a/b for different values of H o , when m=1. 18
- 13. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012 Figure 2. The second mode of dimensionless frequency for longitudinal vibrations versus different values of h=a/b for different values of H o , when m=1. Figure 3. The second mode of dimensionless frequency for longitudinal vibrations versus different values of h=a/b for different values of H o , when m=1. 19
- 14. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012 Figure 4. The first three modes of dimensionless frequency of longitudinal vibrations versus different values of h=a/b for H o = 10 7 , when m=1. Figure 5. The first mode of dimensionless frequency of radial vibrations versus different values of h=a/b for different values of H o , when m=0. 20
- 15. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012 Figure 6. The second mode of dimensionless frequency of radial vibrations versus different values of h=a/b for different values of H o , when m=0. Figure 7. The third mode of dimensionless frequency of radial vibrations versus different values of h=a/b for different values of H o , when m=0. 21
- 16. Mathematical Theory and Modeling www.iiste.orgISSN 2224-5804 (Paper) ISSN 2225-0522 (Online)Vol.2, No.9, 2012 Figure 8. The first three modes of dimensionless frequency of radial vibrations versus different values of h=a/b, for H o = 5 × 10 6 , when m=0. Figure 9. The first three modes of dimensionless frequency of axial shear vibrations versus different values of h=a/b, when m=0. 22
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