Eigenfunction Matching for a Finite Floating Elastic Plate using Symmetry

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Introduction

We show here a solution for a finite Floating Elastic Plate on Finite Depth. The simpler solution for a Semi-Infinite Elastic Plate describes many of the ideas here in more detail. We use Symmetry in Two Dimensions.

Equations

We consider the problem of small-amplitude waves which are incident on finite floating elastic plate occupying water surface for [math]-L\ltx\ltL[/math]. These equations are derived in Floating Elastic Plate The submergence of the plate is considered negligible. We assume that the problem is invariant in the [math]y[/math] direction. We also assume that the plate edges are free to move at each boundary, although other boundary conditions could easily be considered using the methods of solution presented here. We begin with the Frequency Domain Problem for a semi-infinite Floating Elastic Plates in the non-dimensional form of Tayler 1986 (Dispersion Relation for a Floating Elastic Plate). We also assume that the waves are normally incident (incidence at an angle will be discussed later).

[math] \Delta \phi = 0, \;\;\; -h \lt z \leq 0, [/math]
[math] \partial_z \phi = 0, \;\;\; z = - h, [/math]
[math] \partial_z\phi=\alpha\phi, \,\, z=0,\,x\lt-L,\,\,{\rm or}\,\,x\gtL [/math]
[math] \partial_x^2\left\{\beta(x) \partial_x^2\partial_z \phi\right\} - \left( \gamma(x)\alpha - 1 \right) \partial_z \phi - \alpha\phi = 0, \;\; z = 0, \;\;\; -L \leq x \leq L, [/math]

where [math]\alpha = \omega^2[/math], [math]\beta[/math] and [math]\gamma[/math] are the stiffness and mass constant for the plate respectively. The free edge conditions at the edge of the plate imply

[math] \partial_x^3 \partial_z\phi = 0, \;\; z = 0, \;\;\; x = \pm L, [/math]
[math] \partial_x^2 \partial_z\phi = 0, \;\; z = 0, \;\;\; x = \pm L, [/math]

Method of solution

We use separation of variables in the two regions, [math]-L\ltx\ltL[/math] and [math]x\gtL,x\lt-L[/math].

We express the potential as

[math] \phi(x,z) = X(x)Z(z)\, [/math]

and then Laplace's equation becomes

[math] \frac{X^{\prime\prime}}{X} = - \frac{Z^{\prime\prime}}{Z} = k^2 [/math]

Separation of variables for a free surface

We use separation of variables

We express the potential as

[math] \phi(x,z) = X(x)Z(z)\, [/math]

and then Laplace's equation becomes

[math] \frac{X^{\prime\prime}}{X} = - \frac{Z^{\prime\prime}}{Z} = k^2 [/math]

The separation of variables equation for deriving free surface eigenfunctions is as follows:

[math] Z^{\prime\prime} + k^2 Z =0. [/math]

subject to the boundary conditions

[math] Z^{\prime}(-h) = 0 [/math]

and

[math] Z^{\prime}(0) = \alpha Z(0) [/math]

We can then use the boundary condition at [math]z=-h \, [/math] to write

[math] Z = \frac{\cos k(z+h)}{\cos kh} [/math]

where we have chosen the value of the coefficent so we have unit value at [math]z=0[/math]. The boundary condition at the free surface ([math]z=0 \,[/math]) gives rise to:

[math] k\tan\left( kh\right) =-\alpha \, [/math]

which is the Dispersion Relation for a Free Surface

The above equation is a transcendental equation. If we solve for all roots in the complex plane we find that the first root is a pair of imaginary roots. We denote the imaginary solutions of this equation by [math]k_{0}=\pm ik \,[/math] and the positive real solutions by [math]k_{m} \,[/math], [math]m\geq1[/math]. The [math]k \,[/math] of the imaginary solution is the wavenumber. We put the imaginary roots back into the equation above and use the hyperbolic relations

[math] \cos ix = \cosh x, \quad \sin ix = i\sinh x, [/math]

to arrive at the dispersion relation

[math] \alpha = k\tanh kh. [/math]

We note that for a specified frequency [math]\omega \,[/math] the equation determines the wavenumber [math]k \,[/math].

Finally we define the function [math]Z(z) \,[/math] as

[math] \chi_{m}\left( z\right) =\frac{\cos k_{m}(z+h)}{\cos k_{m}h},\quad m\geq0 [/math]

as the vertical eigenfunction of the potential in the open water region. From Sturm-Liouville theory the vertical eigenfunctions are orthogonal. They can be normalised to be orthonormal, but this has no advantages for a numerical implementation. It can be shown that

[math] \int\nolimits_{-h}^{0}\chi_{m}(z)\chi_{n}(z) \mathrm{d} z=A_{n}\delta_{mn} [/math]

where

[math] A_{n}=\frac{1}{2}\left( \frac{\cos k_{n}h\sin k_{n}h+k_{n}h}{k_{n}\cos ^{2}k_{n}h}\right). [/math]

Separation of variables under the Plate

[math] Z^{\prime\prime} + \kappa^2 Z =0. [/math]

subject to the boundary conditions

[math] Z^{\prime}(-h) = 0 [/math]

and

[math] \left(\beta \kappa^4 + 1 - \alpha\gamma\right)Z^{\prime}(0) = \alpha Z(0) [/math]

(the first term comes from the beam eigenvalue problem, where [math]\partial_x^4 X = \kappa^4 X[/math]). We then use the boundary condition at [math]z=-h \,[/math] to write

[math] Z = \frac{\cos \kappa(z+h)}{\cos \kappa h} [/math]

The boundary condition at the free surface ([math]z=0[/math]) is the Dispersion Relation for a Floating Elastic Plate

[math] \kappa \tan{(\kappa h)}= -\frac{\alpha}{\beta \kappa^{4} + 1 - \alpha\gamma} [/math]

Solving for [math]\kappa \,[/math] gives a pure imaginary root with positive imaginary part, two complex roots (two complex conjugate paired roots with positive imaginary part in most physical situations), an infinite number of positive real roots which approach [math]{n\pi}/{h} \,[/math] as [math]n[/math] approaches infinity, and also the negative of all these roots (Dispersion Relation for a Floating Elastic Plate) . We denote the two complex roots with positive imaginary part by [math]\kappa_{-2} \,[/math] and [math]\kappa_{-1} \,[/math], the purely imaginary root with positive imaginary part by [math]\kappa_{0} \,[/math] and the real roots with positive imaginary part by [math]\kappa_{n} \,[/math] for [math]n[/math] a positive integer. The imaginary root with positive imaginary part corresponds to a reflected travelling mode propagating along the [math]x[/math] axis. The complex roots with positive imaginary parts correspond to damped reflected travelling modes and the real roots correspond to reflected evanescent modes.

Inner product between free surface and elastic plate modes

[math] \int\nolimits_{-h}^{0}\phi_{n}(z)\psi_{m}(z) d z=B_{mn} [/math]

where

[math] B_{mn}=\frac{k_{n}\sin k_{n}h\cos\kappa_{m}h-\kappa_{m}\cos k_{n}h\sin \kappa_{m}h}{\left( \cos k_{n}h\right) \left( \cos \kappa_{m}h\right) \left( k_{n} ^{2}-\kappa_{m}^{2}\right) } [/math]

Symmetric solution

The potential and its derivative must be continuous across the transition from open water to the plate covered region. Therefore, the potentials and their derivatives at [math]x=0[/math] have to be equal. We also truncate the sum at [math]N[/math] being careful that we have two extra modes on the plate covered region to satisfy the edge conditions. We use Symmetry in Two Dimensions and we express the potential as

[math] \phi = e^{-k_0 (x+L)}\phi_{0}\left( z\right) + \sum_{m=0}^{N} a_{m}^{s} e^{k_n (x+L)}\phi_{m}\left( z\right),\,\,x\lt-L [/math]

[math] \phi =\sum_{m=-2}^{N}b_{m}^{s}\frac{\cosh(\kappa_n x)}{\cosh(\kappa_n L)}\psi_{m}(z),\,\,-L\leq x\leq 0 [/math]

When we equate the potential and its derivative at [math]x=-L[/math] we obtain

[math] \phi_{0}\left( z\right) + \sum_{m=0}^{N} a_{m}^{s} \phi_{m}\left( z\right) =\sum_{m=-2}^{N}b_{m}^{s}\psi_{m}(z) [/math]

and

[math] -k_{0}\phi_{0}\left( z\right) +\sum _{m=0}^{N} a_{m}^{s}k_{m}\phi_{m}\left( z\right) =-\sum_{m=-2}^{N}b_{m}^{s}\kappa_{m}\tanh(\kappa_m h) \psi _{m}(z) [/math]

for each [math]N[/math]. We solve these equations by multiplying both equations by [math]\phi_{l}(z)\,[/math] and integrating from [math]-h[/math] to [math]0[/math] to obtain:

[math] A_{0}\delta_{0l}+a_{l}^{s}A_{l} =\sum_{m=-2}^{N}b_{m}^{s}B_{ml},\,\,0 \leq l \leq N [/math]

and

[math] -k_{0}A_{0}\delta_{0l}+a_{l}^{s}k_{l}A_l =-\sum_{m=-2}^{N}b_{m}^{s}\kappa_{m}\tanh(\kappa_m L) B_{ml},\,\,0 \leq l \leq N [/math]

If we multiply the first equation by [math]k_l[/math] and subtract the second equation we obtain

[math] 2k_{0}A_{0}\delta_{0l} =\sum_{m=-2}^{N}b_{m}^{s}(k_l + \tanh(\kappa_m L)\kappa_{m})B_{ml} [/math]

Finally, we need to apply the conditions at the edge of the plate to give us two further equations,

[math] \partial_x^2\partial_z\phi = - \sum_{m=-2}^{N}b_{m}^{s} \kappa_m^3 \tan\kappa_m h = 0 [/math]

and

[math] \partial_x^3\partial_z\phi = \sum_{m=-2}^{N}b_{m}^{s} \kappa_m^4 \tanh(\kappa_m L)\tan\kappa_m h = 0 [/math]

Waves Incident at an Angle

We can consider the problem when the waves are incident at an angle [math]\theta[/math]. When a wave in incident at an angle [math]\theta [/math] we have the wavenumber in the [math]y[/math] direction is [math]k_y = \sin\theta k_0[/math] where [math]k_0[/math] is as defined previously (note that [math]k_y[/math] is imaginary).

This means that the potential is now of the form [math]\phi(x,y,z)=e^{k_y y}\phi(x,z)[/math] so that when we separate variables we obtain

[math] k^2 = k_x^2 + k_y^2 [/math]

where [math]k[/math] is the separation constant calculated without an incident angle.

This means that the potential is now of the form [math]\phi(x,y,z)=e^{k_y y}\phi(x,z)[/math] so that when we separate variables we obtain

Therefore the potential can be expanded as

[math] \phi(x,z)=e^{-\hat{k}_0x}\phi_0(z)+\sum_{m=0}^{\infty}a_{m}^{s}e^{\hat{k}_{m}x}\phi_{m}(z), \;\;x\lt-L [/math]

and

[math] \phi(x,z)=\sum_{m=-2}^{\infty}b_{m}^{s} \frac{\cosh(\hat{\kappa}_{m}x)}{\cosh(\hat{\kappa}_{m} L)} \psi_{m}(z), \;\;-L \leq x \leq 0 [/math]

where [math]\hat{k}_{m} = \sqrt{k_m^2 + k_y^2}[/math] and [math]\hat{\kappa}_{m} = \sqrt{\kappa_m^2 + k_y^2}[/math] where we always take the positive real root or the root with positive imaginary part.

The edge conditions are also different and are

[math]\begin{matrix} \left(\frac{\partial^3}{\partial x^3} - (2 - \nu)k^2_y\frac{\partial}{\partial x}\right) \frac{\partial\phi}{\partial z}= 0, \end{matrix}[/math]

and

[math]\begin{matrix} \left(\frac{\partial^2}{\partial x^2} - \nu k^2_y\right)\frac{\partial\phi}{\partial z} = 0, \end{matrix}[/math]

where [math]\nu[/math] is Poisons ratio.

We can expend these edge conditions, which respectively gives

[math] -\sum_{m=-2}^{\infty}b_{m}\kappa_m (\hat{\kappa}_m^3-\hat{\kappa}_m k_y^2(2-\nu))\tanh(\hat{\kappa}_m L)\tan \kappa_m h=0 [/math]

and

[math] -\sum_{m=-2}^{\infty}b_{m}\kappa_m (\hat{\kappa}_m^2-k_y^2\nu))\tan \kappa_m h=0 [/math]

The equations are derived almost identically to those above and we obtain

[math] A_{0}\delta_{0l}+a_{l}^{s}A_{l} =\sum_{m=-2}^{\infty}b_{m}^{s}B_{ml} [/math]

and

[math] -\hat{k_{0}}A_{0}\delta_{0l}+a_{l}^{s}\hat{k}_{l}A_l =-\sum_{m=-2}^{\infty}b_{m}^{s}\hat{\kappa}_{m}\tanh(\kappa_m L)B_{ml} [/math]

and these are solved exactly as before.

Anti-symmetric solution

The anti-symmetric potential can be expanded as

[math] \phi(x,z)=e^{-\hat{k}_0 x}\phi_0(z)+\sum_{m=0}^{\infty}a_{m}^{a}e^{\hat{k}_{m}x}\phi_{m}(z), \;\;x\lt-L [/math]

and

[math] \phi(x,z)=\sum_{m=-2}^{\infty}b_{m}^{a} \frac{\sinh(\hat{\kappa}_{m} x)}{\sinh(-\hat{\kappa}_{m} L)} \psi_{m}(z), \;\;-L \leq x \leq 0 [/math]

The edge conditions are

[math] \sum_{m=-2}^{\infty}b_{m}\kappa_m (\hat{\kappa}_m^3-\hat{\kappa}_m k_y^2(2-\nu))\coth(\hat{\kappa}_m L)\tan \kappa_m h=0 [/math]

and

[math] -\sum_{m=-2}^{\infty}b_{m}\kappa_m (\hat{\kappa}_m^2-k_y^2\nu))\tan \kappa_m h=0 [/math]

The equations are derived almost identically to those above and we obtain

[math] A_{0}\delta_{0l}+a_{l}^{s}A_{l} =\sum_{m=-2}^{\infty}b_{m}^{s}B_{ml} [/math]

and

[math] -\hat{k_{0}}A_{0}\delta_{0l}+a_{l}^{s}\hat{k}_{l}A_l =-\sum_{m=-2}^{\infty}b_{m}^{s}\hat{\kappa}_{m}\coth(\kappa_m L)B_{ml} [/math]

and these are solved exactly as before.

Matlab Code

A program to calculate the coefficients for the semi-infinite dock problems can be found here finite_plate_symmetry.m

Additional code

This program requires