A non-linear finite element method on unstructured meshes for added resistance in waves

ABSTRACT

In this work a finite element method (FEM) is proposed to solve the problem of estimating the added resistance of a ship in waves in the time domain and using unstructured meshes. Two different schemes are used to integrate the corresponding free surface kinematic and dynamic boundary conditions: the first one based on streamlines integration (SLI); and the second one based on the Streamline-Upwind Petrov-Galerking (SUPG) stabilization. The proposed numerical schemes have been validated in different test cases, including towing tank tests with monochromatic waves. The results obtained in this work show the suitability of the present method to estimate added resistance in waves in a computationally affordable manner.

Keywords: Added resistance in waves, FEM, unstructured mesh, potential flow.

1. Introduction

In order to get a good prediction of the total resistance of a ship in a seaway the added resistance in waves has to be taken into account. And although the added resistance in waves is a second order component, it may reach up to 40% of the total average resistance for some specific wave frequencies where wave radiation increases.

Despite of the importance of the added resistance in waves and its impact on the long term performance of a ship, there are not many works in the literature coping with this problem using computational methods. Some formulation have been derived by different authors as an extension of the mean drift force induced by waves in the presence of a water current (Maruo 1957; Journée 1992). These approaches basically modify damping and added mass coefficients, as well as the mean drift forces, to account for the current effect. However, convective terms in the free surface boundary conditions are neglected, limiting this approach to low Froude numbers. A more sophisticated approach is to solve the three dimensional potential flow problem in the frequency domain using the boundary element method (BEM), and obtain the added resistance using Maruo’s approach thereafter (Maruo 1960; Maruo 1963; Liu at al. 2011). However, Maruo’s approach is still limited to low Froude numbers, since it does not account for the free surface convective terms either. Few works can be found trying to solve the added resistance in waves in the time domain considering the convective terms in the free surface boundary condition and using potential flow (Joncquez 2009; Seo et al. 2013; Afshar 2014; Park et al. 2016). The latter approaches are based on the BEM, consider linearized convective terms, and are constrained to structured meshes.

Non-linear viscous CFD solvers have also been applied to analyze details of the added resistance in waves (Sadat-Hosseini et al. 2013; el Moctar et al. 2015;Tezdogan et al. 2015; Kim et al. 2017a; kim et al. 2017b; Kim et al. 2017c; Ozdemir and Barlas 2017; Hizir et al. 2018). Recently Sigmund and el Moctar (2018) carried out state of the art numerical and experimental investigations on four types of ships using the finite volume method. The effect on added resistance of the ship's speed, wave steepness, skin friction and diffraction-radiation was analyzed in detail. Among other findings, it was found that:  calm water and added resistance must be computed on the same numerical grid; radiation forces are more influenced by the ship's speed than by the diffraction forces; in short waves and at model scale frictional resistance accounts for some 20% of the total added resistance, while this percentage is not as high for full scale; and, finally, that the assumption of a quadratic dependence of added resistance on wave amplitude holds for moderate and long waves, while it does not in short waves because wave diffraction is dominant. However, since the use of CFD tools is computationally expensive, its application is limited to research analysis. On the other hand, potential flow solver are more suitable to evaluate systematically a large number of navigation conditions.

The main motivation of this work is the development of a new time-domain computational model capable of solving the wave making and added resistance problem efficiently. This can be achieved by offering am accurate approach not subject to the use of structured meshes.

The proposed method is based on potential flow and applies the free surface boundary conditions on the mean water level for computational efficiency. The main novelties of the model are the use of the Finite Element Method (FEM) on unstructured meshes (Servan-Camas and Garcia-Espinosa 2013, Garcia-Espinosa et al. 2015; Servan-Camas 2016; Oñate et al. 2018) in the context of potential flow. The proposed numerical scheme is derived using a non-linear (NL) formulation for the convective terms, although the Neumann-Kelvin (NK) and double-body (DB) flow linearizations have been analyzed as well.

The first scheme proposed for integrating the free surface boundary conditions is based on computing the convective term as a derivative along the streamlines. To this end a third order finite difference (FD) scheme using three points upwind and one point downwind has been tailored. The second scheme proposed is based on the FEM with Streamline-Upwind Petrov-Galerkin (SUPG) stabilization (Brooks and Hughes 1982).

2. Mathematical models for wave resistance problems

2.1 Problem statement

We consider the first-order diffraction-radiation problem of a body moving on the horizontal plane. Potential flow is assumed and the problem is formulated in terms of the velocity potential and free surface elevation. The following assumptions are made on the order of magnitude of the velocity components and free surface elevation:

${\textstyle \left|{\boldsymbol {V}}_{b}\sim O(1)\right|}$ , ${\textstyle \left|{\boldsymbol {u}}\sim O(1)\right|}$ , ${\textstyle {\varphi }_{x}\sim O(1)}$, ${\textstyle {\varphi }_{y}\sim O(1)}$,	(1)
${\textstyle {\varphi }_{z}\sim O(\epsilon )}$, ${\textstyle {\varphi }_{\alpha \beta }\sim O(\epsilon )}$, ${\textstyle {\xi }_{x}\sim O(\epsilon )}$, ${\textstyle {\xi }_{y}\sim O(\epsilon )}$ ,

where ${\textstyle \varphi }$ the velocity potential, ξ is is the free surface elevation, ${\textstyle {\boldsymbol {V}}_{b}}$ is the forward speed of the moving body and ${\textstyle {\boldsymbol {u}}}$ is the uniform water current vector. The velocity potential and free surface elevation are split into incident and diffraction-radiation components:

${\textstyle \varphi =\psi +\phi }$ ,	(2)
${\textstyle \xi =\zeta +\eta }$ ,	(3)

where ${\textstyle \phi }$ and ${\textstyle \eta }$ are the diffraction-radiation velocity potential and free surface elevation, and ${\textstyle \,\psi }$ and ${\textstyle \zeta }$ are the incident wave potential and free surface elevation (modeled as a set of Airy waves).

2.2 Governing equations in a moving frame of reference

The governing equations are solved in a frame of reference fixed to the moving body. Let the two dimensional movement of the local frame be defined by the horizontal velocity ${\textstyle {\boldsymbol {V}}_{b}}$ (see Figure 1). This frame of reference is assumed to match the global frame at time zero. For an observer sitting on the ship the flow field around is given by the relative motion ${\textstyle {\boldsymbol {U}}_{b}{\boldsymbol {=u-}}{\boldsymbol {V}}_{b}}$. Then the first-order diffraction-radiation equations in the local frame of reference are (see Servan-Camas 2016):

$\Delta \phi =0$ ${\textstyle in\,\Omega }$ ,	(4)
${\frac {\partial \phi }{\partial t}}+{\boldsymbol {U}}_{b}\cdot {\nabla }_{h}\phi +{\frac {1}{2}}{\nabla }_{h}\phi {\cdot \nabla }_{h}\phi +$${\nabla }_{h}\psi {\cdot \nabla }_{h}\phi +g\eta =0$ ${\textstyle on\,z=0}$,	(5)
${\frac {\partial \eta }{\partial t}}+\left({\boldsymbol {U}}_{b}+\right.$$\left.{\nabla }_{h}\phi \right)\cdot {\nabla }_{h}\eta +{\nabla }_{h}\phi \cdot {\nabla }_{h}\zeta -$${\frac {\partial \phi }{\partial z}}=0$ ${\textstyle on\,z=0}$,	(6)
$\nabla \phi \cdot {\boldsymbol {n}}_{p}=-\left({\mathit {\boldsymbol {v}}}_{p}+\right.$$\left.{\boldsymbol {u}}+{\mathit {\boldsymbol {v}}}_{\psi }\right)\cdot {\boldsymbol {n}}_{p}$ ${\textstyle on\,{S}_{B}^{0}}$,	(7)
${\frac {\partial \phi }{\partial z}}=0$ ${\textstyle on\,z=-H}$,	(8)

where ${\textstyle {\mathit {\boldsymbol {v}}}_{\psi }=\nabla \psi }$ , ${\textstyle {S}_{B}^{0}}$ is the body surface below ${\textstyle z=}$$0$, ${\textstyle {\mathit {\boldsymbol {v}}}_{p}}$ is the velocity of a point P on ${\textstyle {S}_{B}^{0}}$, and ${\textstyle H}$ is the water depth The pressure induced by diffracted and radiated waves is

${\textstyle {P}_{p}=-\rho \left({\frac {\partial \phi }{\partial t}}+\right.}$$\left.\left({\boldsymbol {U}}_{b}+{\nabla }_{h}\phi +{\nabla }_{h}\psi \right)\cdot {\nabla }_{h}\phi {\mathit {\boldsymbol {\,}}}-\right.$$\left.{\frac {1}{2}}{\nabla }_{h}\phi \cdot {\nabla }_{h}\phi \right)$ ${\textstyle in\,\Omega }$ .

(9)

Figure 1: Global and local frame of reference.

2.3 Flow linearization

The previous governing equations have been obtained under the assumption ${\textstyle \nabla \phi \sim O(1)}$. Then the free surface boundary conditions remain non-linear and can be written as follows

${\frac {\partial \phi }{\partial t}}+\left({\boldsymbol {U}}_{b}+\right.$$\left.{\nabla }_{h}\phi \right)\cdot {\nabla }_{h}\phi -{\frac {1}{2}}{\nabla }_{h}\phi {\cdot \nabla }_{h}\phi +$${\nabla }_{h}\psi {\cdot \nabla }_{h}\phi +g\eta =0$ ${\textstyle on\,z=0}$,	(10)
${\frac {\partial \eta }{\partial t}}+\left({\boldsymbol {U}}_{b}+\right.$$\left.{\nabla }_{h}\phi \right)\cdot {\nabla }_{h}\eta +{\nabla }_{h}\phi \cdot {\nabla }_{h}\zeta -$${\frac {\partial \phi }{\partial z}}=0$ ${\textstyle on\,z=0}$,	(11)

where ${\textstyle {\boldsymbol {U}}_{b}+{\nabla }_{h}\phi }$ represents the convective velocity and must be updated every iteration to account for the variations of ${\textstyle {\boldsymbol {U}}_{b}}$ and ${\textstyle {\nabla }_{h}\phi }$ . Retaining this assumption allows for simulating flows where ${\textstyle {\boldsymbol {U}}_{\boldsymbol {b}}}$ is not steady. However, linearization of the convective velocity is a common practice when ${\textstyle {\boldsymbol {U}}_{b}}$ is steady and under assumptions of low speed or slender bodies. Two commonly used linearizations are:

The NK linearization: assumes ${\textstyle {\nabla }_{h}\phi \sim O(\epsilon )}$. Then the convective velocity becomes the apparent velocity ${\textstyle {\boldsymbol {U}}_{b}{\boldsymbol {=u-}}{\boldsymbol {V}}_{b}}$.

The DB linearization: assumes ${\textstyle {\nabla }_{h}\phi ={\nabla }_{h}{\phi }^{DB}+}$${\nabla }_{h}{\phi }^{\ast }$ with ${\textstyle {\nabla }_{h}{\phi }^{DB}\sim O(1)}$ and ${\textstyle {\nabla }_{h}{\phi }^{\ast }\sim O(\epsilon )}$ . The ${\textstyle {\nabla }_{h}{\phi }^{DB}}$ flow field is obtained from the double-body approximation (see Servan-Camas 2016).

2.4 Second-order pressure correction over body

A second-order correction on the pressure calculation is proposed in order to better estimate hydrodynamic loads. The idea is to retain second-order terms depending on the first-order solution. Although this will not provide a full second-order solution, it will retain the terms contributing to mean drift loads ( ${\textstyle {\boldsymbol {U}}_{b}=}$$0$), and added resistance in waves ( ${\textstyle {\boldsymbol {U}}_{b}{\mathit {\boldsymbol {\not =}}}0}$). The second-order pressure correction is:

${P}_{p}^{c\left(2\right)}\,=-\rho {\mathit {\boldsymbol {r}}}_{p}^{1}\cdot \nabla \left({P}_{p}^{I}+\right.$$\left.{P}_{p}^{DR}\right)-\rho \left({\frac {1}{2}}{\phi }_{z}{\phi }_{z}+{\phi }_{z}{\psi }_{z}+\right.$$\left.{\frac {1}{2}}\nabla \psi \cdot \nabla \psi \right),$

(12)

where ${\textstyle {P}_{p}^{I}}$ and ${\textstyle {P}_{p}^{DR}}$ are pressures induced by the incident and diffracted-radiated waves respectively, ${\textstyle {\mathit {\boldsymbol {r}}}_{p}^{1}}$ is the first-order displacement of a point P over the body surface, and ${\textstyle {P}_{p}^{c\left(2\right)}}$ is the pressure correction term. The first term of the right hand side account for the pressure variation due to first order movements, and the second term accounts for second-order terms depending on first-order terms.

2.5 Second-order pressure correction on waterline

The movements of a ship and the free surface elevation modify the wetted surface. In order to take into account this change, a linear pressure is assumed from the waterline to the free surface (see Figure 2):

${\textstyle {P}_{p}^{wl}={P}_{p}^{I}+{P}_{p}^{DR}-\rho g{r}_{pz}}$,	(13)
${P}_{p}^{wl\left(2\right)}\,\left(z\right)={P}_{p}^{wl}-\left({P}_{p}^{wl}-\right.$$\left.{P}_{p}^{fs}\right){\frac {z}{\xi -{r}_{pz}}},$	(14)

where ${\textstyle {P}_{p}^{I}}$ and ${\textstyle {P}_{p}^{DR}}$ are evaluated at z=0, ${\textstyle {P}_{p}^{wl}}$ is the first-order pressure at z=0, and ${\textstyle {P}_{p}^{wl\left(2\right)}}$ represents the vertical pressure distribution over the water line (see Servan-Camas 2016).

Figure 2: Pressure estimation at the waterline area.

3. Numerical schemes

3.1 Problem statement

Let ${\textstyle {Q}_{h}^{\ast }}$ be the finite element (FE) space of interpolating functions, defined in the usual manner. From this space we can construct the subspace ${\textstyle {Q}_{h,\phi }}$ that incorporates the Dirichlet conditions for the velocity potential ${\textstyle \phi }$ . The space of test functions, denoted by ${\textstyle {Q}_{h}}$, is constructed as ${\textstyle {Q}_{h,\phi }}$, but with functions vanishing on the boundary where the Dirichlet conditions are imposed. Then the discrete variational finite element problem associated with the Eqs. (27)-(31) can be written as follows (Belibassakis et al. 2013): Find ${\textstyle \left[{\phi }_{h}\right]\in {Q}_{h,\phi }}$, by solving

${\textstyle \int _{\Omega }^{}\nabla {\nu }_{h}\cdot \nabla {\phi }_{h}d\Omega =}$$\int _{{\Gamma }^{B}}^{}{\nu }_{h}\cdot {\hat {\phi }}_{n}^{B}d\Gamma +\int _{{\Gamma }^{R}}^{}{\nu }_{h}\cdot {\hat {\phi }}_{n}^{R}d\Gamma +\int _{{\Gamma }^{{Z}_{o}}}^{}{\nu }_{h}\cdot {\hat {\phi }}_{n}^{{Z}_{o}}d\Gamma \quad \,\forall {\nu }_{h}\in {Q}_{h}$,

(15)

where ${\textstyle {\hat {\phi }}_{n}^{B}}$, ${\textstyle {\hat {\phi }}_{n}^{R}}$, ${\textstyle {\hat {\phi }}_{n}^{{Z}_{o}}}$ are the potential normal gradients corresponding to the Neumann boundary conditions on bodies, radiation boundary and free surface, respectively. At this point it is useful to introduce the associated matrix form (Zienkiewicz et al. 2005a)

${\textstyle {\overline {\overline {\boldsymbol {L}}}}{\boldsymbol {\phi }}=}$${\boldsymbol {b}}^{{Z}_{0}}+{\boldsymbol {b}}^{B}+{\boldsymbol {b}}^{R}$,

(16)

where ${\textstyle {\overline {\overline {\boldsymbol {L}}}}}$ is the standard FE Laplacian matrix, and ${\textstyle {\boldsymbol {b}}^{{Z}_{0}}}$ is a vector accounting for the right hand side of the dynamic condition of the free surface, and ${\textstyle {\boldsymbol {b}}^{B}}$ and ${\textstyle {\boldsymbol {b}}^{R}}$ are the vectors resulting from integrating the other boundary condition terms.

Two different schemes have been developed to integrate the free surface boundary conditions (Eq. (10) and Eq. (11)): one based on FD streamline integration (FD-SLI), and the other based on FEM with SUPG stabilization scheme (FEM-SUPG). Both schemes have been tailored to account for the non-linear convective terms and to be used on unstructured meshes.

3.2 FD-SLI

The first-order free surface boundary conditions can be written in a general form as follows:

${\frac {\partial \phi }{\partial t}}+{\boldsymbol {U}}\cdot {\nabla }_{h}\phi +{\frac {{P}_{fs}}{\rho }}+g\eta +R=$$0$ ${\textstyle on\,z=0}$,	(17)
${\frac {\partial \eta }{\partial t}}+{\boldsymbol {U}}\cdot {\nabla }_{h}\eta -{\frac {\partial \phi }{\partial z}}+S=$$0$ ${\textstyle on\,z=0}$,	(18)

where ${\textstyle R}$ and ${\textstyle S}$ represent remaining terms depending on the linearization used. The numerical schemes adopted for solving the kinematic-dynamic free surface boundary conditions are based on Adams-Bashforth-Moulton schemes, using an explicit scheme for the kinematic condition, and an implicit one for the dynamic condition. Then ${\textstyle {\phi }^{n+1}}$ is imposed as a Dirichlet boundary condition. The schemes read as follows:

${\textstyle {\phi }^{n+1}+\Delta t{\left({\mathit {\boldsymbol {U}}}\cdot {\nabla }_{h}\phi \right)}^{n+1}=}$${\phi }^{n}-\Delta t\left({\frac {1}{\rho }}{P}_{fs}^{n+1}-g{\eta }^{n+1}-{R}^{n+1}\right)$ ${\textstyle on\,z=0}$,	(19)
${\eta }^{n+1}={\eta }^{n}-\Delta t{\left({\boldsymbol {U}}\cdot {\nabla }_{h}\eta \right)}^{n}+$$\Delta t\left({\phi }_{z}^{n}-{S}^{n}\right)$ ${\textstyle on\,z=0}$,	(20)

where ${\textstyle {\boldsymbol {U}}}$ is the convective velocity and the convective terms are evaluated by differentiating along streamlines as:

${\left({\boldsymbol {U}}\cdot {\nabla }_{h}\phi \right)}^{n+1}={\left|{\mathit {\boldsymbol {U}}}\right|}^{n+1}{\partial }_{L}{\phi }^{n+1}\,,$	(21)
${\left({\boldsymbol {U}}\cdot {\nabla }_{h}\eta \right)}^{n}={\left|{\mathit {\boldsymbol {U}}}\right|}^{n}{\partial }_{L}{\eta }^{n}\,,$

where ${\textstyle {\partial }_{L}}$ denotes the derivative along the streamline. This streamline derivative is estimated using a two points upstream and one point downstream FD operator. Figure 3 shows the tracing of the streamline at node 0. The left (-1) and forward left (-2) points are upstream points, while the right (1) point corresponds to the downstream point. Then the streamline differential operator reads as:

${\partial }_{L}{\phi }_{0}={w}_{1}{\phi }_{1}+{w}_{0}{\phi }_{0}+{w}_{-1}{\phi }_{-1}+$${w}_{-2}{\phi }_{-2},$	(22)
${\partial }_{L}{\eta }_{0}={w}_{1}{\eta }_{1}+{w}_{0}{\eta }_{0}+{w}_{-1}{\eta }_{-1}+$${w}_{-2}{\eta }_{-2},$

where ${\textstyle {\phi }_{1}}$, ${\textstyle {\phi }_{-1}}$, ${\textstyle {\phi }_{-2}}$ are interpolated between ${\textstyle \left({\phi }_{1a},{\phi }_{1b}\right)}$ , ${\textstyle \left({\phi }_{-1a},{\phi }_{-1b}\right)}$ , and ${\textstyle \left({\phi }_{-2a},{\phi }_{-2b}\right)}$ respectively. In matrix form, the resulting scheme can be written as:

${\textstyle \left({\overline {\overline {\mathit {\boldsymbol {I}}}}}+\right.}$$\left.\Delta t{\overline {\overline {\boldsymbol {W}}}}^{\mathit {\boldsymbol {n+1}}}\right){\mathit {\boldsymbol {\phi }}}^{n+1}=$${\overline {\overline {\mathit {\boldsymbol {I}}}}}\left({\mathit {\boldsymbol {\phi }}}^{n}-\right.$$\left.\Delta t\left({\frac {1}{\rho }}{\mathit {\boldsymbol {P}}}_{fs}^{n+1}-g{\mathit {\boldsymbol {\eta }}}^{n+1}-\right.\right.$$\left.\left.{\mathit {\boldsymbol {R}}}^{n+1}\right)\right)$ ${\textstyle on\,z=0}$,

(23)

${\overline {\overline {\mathit {\boldsymbol {I}}}}}{\mathit {\boldsymbol {\,\eta }}}^{n+1}=$$\left({\overline {\overline {\mathit {\boldsymbol {I}}}}}-\Delta t{\overline {\overline {\boldsymbol {W}}}}^{\mathit {\boldsymbol {n}}}\right){\mathit {\boldsymbol {\,\eta }}}^{n}+$$\Delta t\left({\mathit {\boldsymbol {\phi }}}_{z}^{n}-{\boldsymbol {S}}^{n}\right)$ ${\textstyle on\,z=0}$,

(24)

where ${\textstyle {\overline {\overline {\boldsymbol {W}}}}}$ and ${\textstyle {\overline {\overline {\mathit {\boldsymbol {I}}}}}}$ are the streamline convective and identity matrices respectively. The stencils are tailored using Taylor series expansion to get a third-order FD scheme along the streamline.

The associated matrix form to the FE formulation for the governing equations is:

${\textstyle {\overline {\overline {{\boldsymbol {L}}^{SL}}}}{\boldsymbol {\phi }}=}$${\boldsymbol {b}}^{SL}+{\boldsymbol {b}}^{B}+{\boldsymbol {b}}^{R}$,

(25)

where ${\textstyle {\overline {\overline {{\boldsymbol {L}}^{SL}}}}}$ is the standard Laplacian matrix modified to account for the left hand side of Eq.(23), ${\textstyle {\boldsymbol {b}}^{SL}}$ is a vector containing the right hand side of Eq. (23), and ${\textstyle {\boldsymbol {b}}^{B}}$ and ${\textstyle {\boldsymbol {b}}^{R}}$ are the vectors resulting from integrating the other boundary condition terms.

Figure 3: SLI discretization

3.3 FEM-SUPG

Alternatively a FEM-SUPG (Hughes and Mallet 1986) has been also developed for integrating the free surface boundary conditions. The dynamic and kinematic boundary conditions can be seen as convective-transport equations of the form:

${\frac {\partial \chi }{\partial t}}+{\boldsymbol {U}}\cdot {\nabla }_{h}\chi +Q=0.$

(26)

The standard FE problem associated to the above equation is

${\textstyle \forall i\,\int _{\Omega }^{}{N}^{i}\,\left({N}^{j}{\frac {\partial {\chi }_{j}}{\partial t}}+{\boldsymbol {U}}\cdot {\nabla }_{h}{N}^{j}{\chi }_{j}+{N}^{j}{Q}_{j}\right)d\sigma =}$$0,$

(27)

where ${\textstyle {N}^{i}\,}$ is the corresponding shape function associated to the mesh node ${\textstyle i}$ and ${\textstyle {\chi }_{j}}$ and ${\textstyle {Q}_{j}}$ represent the values of ${\textstyle {\chi }_{h}}$ and ${\textstyle {Q}_{h}}$ at node ${\textstyle j}$, respectively. The above equation is discretized in time as follows:

$\forall i\,\int _{\Omega }^{}{N}^{i}{N}^{j}{\frac {{{\chi }_{j}}^{n+1}-{{\chi }_{j}}^{n}}{\Delta t}}d\sigma +$$\,\int _{\Omega }^{}{N}^{i}\left({\boldsymbol {U}}^{n+\theta }\cdot {\nabla }_{h}{N}^{j}\right){{\chi }_{j}}^{n+\theta }d\sigma +$$\,\int _{\Omega }^{}{{N}^{i}N}^{j}{Q}_{j}^{n+\theta }d\sigma =0,$

(28)

where ${\textstyle {A}^{n+\theta }=\left(1-\theta \right){A}^{n}+}$$\theta {A}^{n+1}$. It is well known that the numerical solution of the previous equation may show spurious oscillations (Zienkiewicz et al. 2005b; Donea and Huerta 2003). Hence the SUPG formulation is used to introduce the necessary stabilization. The resulting scheme is

$\forall i\,\,\left[\int _{\Omega }^{}{N}^{i}{N}^{j}d\sigma +\sum _{e}^{}{\frac {{h}_{e}}{2\left|{\left({\hat {{\boldsymbol {U}}^{e}}}\right)}^{n+\theta }\right|}}\int _{{\Omega }^{e}\,}^{}\left({\left({\boldsymbol {U}}^{e}\right)}^{n+\theta }\cdot {\nabla }_{h}{N}^{i}\right){N}^{j}d\sigma \right]\left({\chi }_{j}^{n+1}-\right.$$\left.{\chi }_{j}^{n}\right)$ $+\Delta t\,\left[\int _{\Omega }^{}{N}^{i}\left({\left({\boldsymbol {U}}^{\boldsymbol {e}}\right)}^{n+\theta }\cdot {\nabla }_{h}{N}^{j}\right)d\sigma \right]{\chi }_{j}^{n+\theta }$ $+\Delta t\,\left[\sum _{e}^{}{\frac {{h}_{e}}{2\left|{({\hat {{\boldsymbol {U}}^{e}}})}^{n+\theta }\right|}}\int _{{\Omega }^{e}}^{}\left({\left({\boldsymbol {U}}^{e}\right)}^{n+\theta }\cdot {\nabla }_{h}{N}^{i}\right)\left({\left({\boldsymbol {U}}^{e}\right)}^{n+\theta }\cdot {\nabla }_{h}{N}^{j}\right)d\sigma \right]{\chi }_{j}^{n+\theta }$ $+\Delta t\left[\int _{\Omega }^{}{N}^{i}{N}^{j}d\sigma +\sum _{e}^{}{\frac {{h}_{e}}{2\left|{{\mathit {\boldsymbol {(}}}{\hat {{\boldsymbol {U}}^{e}}}{\mathit {\boldsymbol {)}}}}^{n+\theta }\right|}}\int _{{\Omega }^{e}\,}^{}\left({\left({\boldsymbol {U}}^{e}\right)}^{n+\theta }\cdot {\nabla }_{h}{N}^{i}\right){N}^{j}d\sigma \right]{Q}_{j}^{n+\theta }=$$0.$

(29)

In matrix form:

$\left({\overline {\overline {\mathit {\boldsymbol {M}}}}}+{\overline {\overline {\mathit {\boldsymbol {M}}}}}_{supg}^{n{\mathit {\boldsymbol {+}}}\theta }\right){\mathit {\boldsymbol {\chi }}}^{n+1}{\boldsymbol {+\Delta }}t\left({\overline {\overline {\mathit {\boldsymbol {C}}}}}^{n{\mathit {\boldsymbol {+}}}\theta }+\right.$$\left.{\overline {\overline {\mathit {\boldsymbol {C}}}}}_{supg}^{n{\mathit {\boldsymbol {+}}}\theta }\right){\theta {\mathit {\boldsymbol {\chi }}}}^{n+1}=$ ${\textstyle \left({\overline {\overline {\mathit {\boldsymbol {M}}}}}+\right.}$$\left.{\overline {\overline {\mathit {\boldsymbol {M}}}}}_{supg}^{n+\theta }\right){\mathit {\boldsymbol {\chi }}}^{n}{\boldsymbol {-\Delta }}t\left({\overline {\overline {\mathit {\boldsymbol {C}}}}}^{n{\mathit {\boldsymbol {+}}}\theta }+\right.$$\left.{\overline {\overline {\mathit {\boldsymbol {C}}}}}_{supg}^{n{\mathit {\boldsymbol {+}}}\theta }\right){\left(1-\theta \right){\mathit {\boldsymbol {\chi }}}}^{n}-$$\left({\overline {\overline {\mathit {\boldsymbol {M}}}}}+{\overline {\overline {\mathit {\boldsymbol {M}}}}}_{supg}^{n+\theta }\right){\mathit {\boldsymbol {Q}}}^{n+\theta },$

(30)

Where

${\left({U}^{e}\right)}^{n+\theta }=\sum _{{k}_{e}}^{}{N}^{{k}_{e}}{U}_{{k}_{e}}^{n+\theta }$ ${\overline {\overline {\mathit {\boldsymbol {M}}}}}=\int _{\Omega }^{}{N}^{i}{N}^{j}d\sigma ,$ ${\overline {\overline {\mathit {\boldsymbol {M}}}}}_{supg}^{n+\theta }=\sum _{e}^{}\left[{\frac {{h}_{e}}{2\left|{\left({\hat {{\mathit {\boldsymbol {U}}}^{e}}}\right)}^{n+\theta }\right|}}\int _{{\Omega }^{e}}^{}\left({\left({\mathit {\boldsymbol {U}}}^{e}\right)}^{n+\theta }\cdot {\nabla }_{h}{N}^{i}\right){N}^{j}d\sigma \right],$ ${\overline {\overline {\mathit {\boldsymbol {C}}}}}^{n+\theta }=\sum _{e}^{}\int _{{\Omega }^{e}}^{}{N}^{i}\left({\mathit {\boldsymbol {U}}}_{e}^{n+\theta }\cdot {\nabla }_{h}{N}^{j}\right),$ ${\overline {\overline {\mathit {\boldsymbol {C}}}}}_{supg}^{n+\theta }=\sum _{e}^{}\left[{\frac {{h}_{e}}{2\left|{\left({\hat {{\mathit {\boldsymbol {U}}}^{e}}}\right)}^{n+\theta }\right|}}\int _{{\Omega }^{e}}^{}\left({\left({\mathit {\boldsymbol {U}}}^{e}\right)}^{n+\theta }\cdot {\nabla }_{h}{N}^{i}\right)\left({\mathit {\boldsymbol {U}}}_{e}^{n+\theta }\cdot {\nabla }_{h}{N}^{j}\right)d\sigma \right].$

(31)

The FEM-SUPG dynamic and kinematic boundary conditions become

$\left({\overline {\overline {\mathit {\boldsymbol {M}}}}}+{\overline {\overline {\mathit {\boldsymbol {M}}}}}_{supg}^{n{\mathit {\boldsymbol {+}}}\theta }\right){\mathit {\boldsymbol {\phi }}}^{n+1}{\boldsymbol {+\Delta }}t\left({\overline {\overline {\mathit {\boldsymbol {C}}}}}^{n{\mathit {\boldsymbol {+}}}\theta }+\right.$$\left.{\overline {\overline {\mathit {\boldsymbol {C}}}}}_{supg}^{n{\mathit {\boldsymbol {+}}}\theta }\right){\theta {\mathit {\boldsymbol {\phi }}}}^{n+1}=$ ${\textstyle \left({\overline {\overline {\mathit {\boldsymbol {M}}}}}+\right.}$$\left.{\overline {\overline {\mathit {\boldsymbol {M}}}}}_{supg}^{n+\theta }\right){\mathit {\boldsymbol {\phi }}}^{n}{\boldsymbol {-\Delta }}t\left({\overline {\overline {\mathit {\boldsymbol {C}}}}}^{n{\mathit {\boldsymbol {+}}}\theta }+\right.$$\left.{\overline {\overline {\mathit {\boldsymbol {C}}}}}_{supg}^{n{\mathit {\boldsymbol {+}}}\theta }\right){\left(1-\theta \right){\mathit {\boldsymbol {\phi }}}}^{n}$ ${\textstyle -\left({\overline {\overline {\mathit {\boldsymbol {M}}}}}+\right.}$$\left.{\overline {\overline {\mathit {\boldsymbol {M}}}}}_{supg}^{n+\theta }\right)\left({\frac {1}{\rho }}{\mathit {\boldsymbol {P}}}^{n+\theta }+\right.$$\left.g{\mathit {\boldsymbol {\eta }}}^{n+\theta }+{\mathit {\boldsymbol {R}}}^{n+\theta }\right){\mathit {\boldsymbol {.}}}$	(32)
$\left({\overline {\overline {\mathit {\boldsymbol {M}}}}}+{\overline {\overline {\mathit {\boldsymbol {M}}}}}_{supg}^{n{\mathit {\boldsymbol {+}}}\theta }\right){\boldsymbol {\eta }}^{n+1}{\boldsymbol {+\Delta }}t\left({\overline {\overline {\mathit {\boldsymbol {C}}}}}^{n{\mathit {\boldsymbol {+}}}\theta }+\right.$$\left.{\overline {\overline {\mathit {\boldsymbol {C}}}}}_{supg}^{n{\mathit {\boldsymbol {+}}}\theta }\right){\theta {\boldsymbol {\eta }}}^{n+1}=$ ${\textstyle \left({\overline {\overline {\mathit {\boldsymbol {M}}}}}+\right.}$$\left.{\overline {\overline {\mathit {\boldsymbol {M}}}}}_{supg}^{n+\theta }\right){\boldsymbol {\eta }}^{n}{\boldsymbol {-\Delta }}t\left({\overline {\overline {\mathit {\boldsymbol {C}}}}}^{n{\mathit {\boldsymbol {+}}}\theta }+\right.$$\left.{\overline {\overline {\mathit {\boldsymbol {C}}}}}_{supg}^{n{\mathit {\boldsymbol {+}}}\theta }\right){\left(1-\theta \right){\boldsymbol {\eta }}}^{n}$ ${\textstyle +\left({\overline {\overline {\mathit {\boldsymbol {M}}}}}+\right.}$$\left.{\overline {\overline {\mathit {\boldsymbol {M}}}}}_{supg}^{n{\mathit {\boldsymbol {+}}}\theta }\right)\left({\frac {1}{\rho }}{\mathit {\boldsymbol {\phi }}}_{z}^{n{\mathit {\boldsymbol {+}}}\theta }-\right.$$\left.{\mathit {\boldsymbol {S}}}^{n+\theta }\right){\mathit {\boldsymbol {.}}}$		(33)

In this work an explicit ( ${\textstyle \theta =0}$) and implicit ( ${\textstyle \theta =}$$1$) schemes are used for the kinematic and dynamic conditions respectively. The matrix form associated to the FE formulation of the governing equations is:

${\textstyle {\overline {\overline {{\boldsymbol {L}}^{SUPG}}}}{\boldsymbol {\phi }}=}$${\boldsymbol {b}}^{SUPG}+{\boldsymbol {b}}^{B}+{\boldsymbol {b}}^{R}$,

(34)

where ${\textstyle {\overline {\overline {{\boldsymbol {L}}^{SUPG}}}}}$ is the standard Laplacian matrix modified to account for the left hand side of Eq. (32), ${\textstyle {\boldsymbol {b}}^{SUPG}}$ is a vector accounting for the right hand side of Eq. (32), and ${\textstyle {\boldsymbol {b}}^{B}}$ and ${\textstyle {\boldsymbol {b}}^{R}}$ are the vectors resulting of integrating the other boundary condition terms.

4. Hydrodynamic loads for wave resistance problems

4.1 First-order loads

Hydrodynamic forces and moments are obtained from direct pressure integration over the body surface (Bai and Teng 2013). The body gravity center ( ${\textstyle G}$) will be used as a reference for body movements and moments acting on it. The resulting expressions for forces ( ${\textstyle {\mathit {\boldsymbol {F}}}}$) and moments ( ${\textstyle {\mathit {\boldsymbol {M}}}}$) can be found in (Servan-Camas 2016).

4.2 Second-order correction

Second-order correction loads are obtained by calculating the components of the second-order loads depending on the first-order solution as described in section 2.5 (Figure 2). Integrating the corresponding second-order pressure correction:

${\mathit {\boldsymbol {F}}}_{C}^{(2)}=\int _{{S}_{B}}^{}{P}_{p}^{c\left(2\right)}{\mathit {\boldsymbol {n}}}_{p}ds+$$\int _{{\Gamma }_{wl}}^{}{P}_{p}^{wl\left(2\right)}{\frac {{\mathit {\boldsymbol {n}}}_{p}^{0}}{\sqrt {1-{{n}_{pz}^{0}}^{2}}}}dl,$

(35)

${\mathit {\boldsymbol {M}}}_{C}^{(2)}=\int _{{S}_{B}}^{}{P}_{p}^{c\left(2\right)}{\overset {\rightarrow }{\mathit {\boldsymbol {GP}}}}{\mathit {\boldsymbol {\times }}}{\mathit {\boldsymbol {n}}}_{p}ds+$$\int _{{\Gamma }_{wl}}^{}{P}_{p}^{wl\left(2\right)}{\overset {\rightarrow }{\mathit {\boldsymbol {GP}}}}{\mathit {\boldsymbol {\times }}}{\mathit {\boldsymbol {n}}}_{p}{\frac {{\mathit {\boldsymbol {n}}}_{p}^{0}}{\sqrt {1-{{n}_{pz}^{0}}^{2}}}}dl.$

(36)

The mean value of the longitudinal component of ${\textstyle {\mathit {\boldsymbol {F}}}_{C}^{(2)}}$ has a special meaning in the presence of waves: when ${\textstyle {\mathit {\boldsymbol {U}}}=}$$0$ it becomes the mean drift force due to the waves; and when ${\textstyle {\mathit {\boldsymbol {U}}}\not =0}$ it becomes the added resistance in waves. Additionaly second-order correction of dynamic and hydrostatic loads resulting from the first-order rotation (see Servan-Camas 2016) are also taken into account in this work.

5. Verification and validation

5.1 Wave making resistance of an elliptic pressure distribution

5.1.1 Problem description

Newman and Poole (1962) derived an analytical solution for the wave resistance of a pressure distribution moving with constant forward speed along the free surface of a canal with constant width and depth. This solution was obtained based on a first-order approximation with uniform flow (NK). In particular, an analytical expression for the elliptic pressure distribution was obtained. The main particulars of the elliptic pressure distribution used to validate the present model are given in Table 1:

Table 1: Particulars for elliptic pressure distribution.

Length (L)	1 m
Beam (B)	0.5 m
Water depth (H)	5 m
Channel width (W)	10 m
Free surface pressure ( ${\textstyle {P}_{fs}}$)	1 Pa

The wave resistance is obtained by integrating the pressure distribution over the free surface as follows:

${F}_{W}=-\int _{{S}_{FS}}^{}{P}_{fs}{n}_{x}ds.$

(37)

It is assumed that the pressure distribution moves in the x direction. Then, in order to obtain the wave resistance, it is mandatory to be able to estimate the free surface deformation within the pressure patch.

5.1.2 Convergence analysis

Different unstructured meshes have been used for the numerical calculations. It has been found that refinement at the edge of the pressure distribution is mandatory due to the discontinuity in the pressure and its large influence in the free surface deformation, especially at low Froude numbers where wave lengths are smaller. Table 2 provides the particulars for each mesh and Figure 4 shows a detail of the finest one.

Table 2: Characteristic sizes of the used meshes.

	Pressure patch edge (m)	Pressure patch (m)	Free surface outside (m)	Volume (m)
Mesh 1	0.002	0.02	0.02	0.05
Mesh 2	0.003	0.03	0.03	0.075
Mesh 3	0.004	0.04	0.04	0.1
Mesh 4	0.006	0.06	0.06	0.15
Mesh 5	0.008	0.08	0.08	0.20

Wave resistance was calculated for all the meshes at Froude number Fr=0.2, using the FD-SLI and FEM-SUPG schemes presented in sections 3.2 and 3.3 respectively. Table 3 provides the values of the relative errors. Figure 5 shows the free surface elevation computed for Fr=0.2 with the FEM-SUPG and the finer mesh.

Table 3: Dimensionless wave resistance ${\textstyle {\mathit {\boldsymbol {C}}}_{\mathit {\boldsymbol {w}}}{\mathit {\boldsymbol {=\rho g}}}{\mathit {\boldsymbol {F}}}_{\mathit {\boldsymbol {w}}}{\mathit {\boldsymbol {/(}}}{\mathit {\boldsymbol {P}}}_{\mathit {\boldsymbol {fs}}}^{\mathit {\boldsymbol {2}}}{\mathit {\boldsymbol {B)\,}}}}$ at Fr=0.2.

Analytical ${\textstyle {C}_{w}}$=0.1840		Mesh 5	Mesh 4	Mesh 3	Mesh 2	Mesh 1
Streamline	${C}_{w}$	1.550	1.640	1.730	1.780	1.820
	Error	15.77 %	10.88 %	5.99 %	3.27 %	1.10 %
FEM-SUPG	${C}_{w}$	1.643	1.710	1.775	1.795	1.820
	Error	10.74 %	7.08 %	3.54 %	2.46 %	1.10 %

Figure 4: Detail of the finest mesh for the elliptic pressure patch.

Figure 5: Free surface elevation for elliptic pressure distribution at Fr=0.2.

5.1.3 Verification

The wave making resistance has been calculated for several Froude numbers for the finest mesh using the FD-SLI and FEM-SUPG. Table 4 compares analytical and numerical results. It can be observed that the numerical results are able to reproduce the analytical ones with small errors.

Table 4: Dimensionless wave resistance ${\textstyle {\mathit {\boldsymbol {C}}}_{\mathit {\boldsymbol {w}}}{\mathit {\boldsymbol {\,}}}}$for elliptic pressure distribution.

Fr	${\textstyle {C}_{w}=}$$\rho g{F}_{w}/({P}_{fs}^{2}B)\,$
	FD-SLI	FEM-SUPG	Analytical (Newman and Poole 1962)
0.2	1.82	1.82	1.84
0.3	2.18	2.16	2.18
0.4	1.67	1.65	1.64
0.5	2.73	2.66	2.66

5.2.1 Problem description

The wave making resistance of a Wigley hull is analyzed. Different simulations have been performed considering the NL, NK, and DB free surface conditions. The FD-SLI and FEM-SUPG schemes have been used for integrating the free surface boundary conditions. Wave resistance coefficients with and without second-order correction have been obtained.

The standard Wigley hull with beam to length ratio B/L=0.1 and amidships section coefficient C_m=0.6667 was used. An unstructured mesh was generated with an element size around the ship of 0.01 m. The mesh generated consists of 84351 nodes and 476083 tetrahedral elements (see Figure 6). Only half domain was required due to the symmetry of the problem.

Figure 6: Detail of the mesh generated for the Wigley hull.

5.2.2 Second-order correction and flow linearizations

Figure 7 compares the dimensionless first-order wave making resistance coefficients ${\textstyle {C}_{w1}=}$${F}_{Dx}^{1}/(0.5\rho S{U}^{2})$ and the dimensionless second-order-corrected wave making resistance coefficients ${\textstyle {C}_{w2}=}$$\left({F}_{Dx}^{1}+{F}_{Cx}^{2}\right)/(0.5\rho S{U}^{2})$. They have been obtained using the NL, NK and DB assumptions for the case of a fixed Wigley hull model in still water. The wave making resistance forces ${\textstyle {F}_{Dx}^{1}}$ and ${\textstyle {F}_{Cx}^{2}}$ have been calculated as the longitudinal forces obtained by pressure integration (section 4). It is observed that the increase of resistance due to the second-order correction term is noticeable.

The NK linearization leads to smaller values of wave resistance when compared to the NL and DB approaches, while the NL and DB predict similar results up to Fr=0.3.

Figure 7: Wave resistance for Wigley hull using NL, DB, and NK approximations. Dimensionless first-order wave making resistance ( ${\textstyle {C}_{w1}}$), and dimensionless second-order-corrected wave making resistance ( ${\textstyle {C}_{w2}}$).

5.2.3 Validation

Figure 8 compares the second-order-corrected ${\textstyle {C}_{w2}}$ numerical results obtained in this work with NL flow approximation against several experimental results: ITTC (1984) (collection of experimental data), Shearer and Cross (1965), University of Iowa, University of Tokyo (UT), and the Ship Research Institute of Japan (SRI). The results from Iowa, UT and SRI can be found in Ju (1983). Experimental data shows large dispersion and this might be mainly due to the uncertainty of model testing and the assumption of a constant form factor with speed.

Taking into account the large dispersion of the experimental data a fairly good agreement between the numerical and the experimental results has been obtained. This agreement is better for the higher Froude numbers. Lower Froude numbers require a much finer discretization in order to reproduce the shorter wave pattern. Figure 9 compares the wave profiles at the water line obtained numerically against experimental results. A good agreement is also found in this case.

Figure 8: FD-SLI and FEM-SUPG versus experimental results.

Figure 9: Wave profile over Wigley hull.

5.3.1 Problem description

In this section computed added resistance is compared to that obtained by Journée (1992). Journée carried out an extensive model test campaign measuring the added resistance in waves of four modified Wigley hulls.. The main particulars of the models are given in Table 5.

Table 5: Modified Wigley hulls particulars.

	Wigley I	Wigley II	Wigley III	Wigley IV
Amidships section coefficient Cm	0.9090	0.9090	0.6667	0.6667
Length to breadth ratio, L/B	10	5	10	5
Length L (m)	1	1	1	1
Breadth B (m)	0.1	0.2	0.1	0.2
Draught d (m)	0.0625	0.0625	0.0625	0.0625
Displacement (m3)	0.003504	0.007008	0.002889	0.005778
KG (m)	0.05667	0.0625	0.05667	0.0625
Radius of inertia for pitch, kyy (m)	0.25	0.25	0.25	0.25
Pitch damping (N/(m/s))	$0.02{\sqrt {4{I}_{yy}{K}_{55}}}$	$0.10{\sqrt {4{I}_{yy}{K}_{55}}}$	$0.02{\sqrt {4{I}_{yy}{K}_{55}}}$	$0.02{\sqrt {4{I}_{yy}{K}_{55}}}$

5.3.2 Validation

The added resistance ${\textstyle {R}_{aw}}$ has been estimated by subtracting the second-order-corrected longitudinal force in still water to the average value of the second-order-corrected longitudinal force obtained in the presence of a monochromatic wave. Then the dimensionless wave resistance is calculated as:

${R}_{aw}^{\ast }={\frac {{R}_{aw}}{\rho g{A}^{2}{B}^{2}/L}}\,,$

(38)

where A is the wave amplitude.

Simulations have been carried out with the streamlines and FEM-SUPG scheme using the NL flow approximations. Pitch damping was introduced to model the viscous dissipation effects, and prevent the excessive pitch movement around resonance obtained otherwise (see Table 5). The amount of damping introduced was calibrated to best fit the RAOs response across all Froude numbers tested.

Journée (1992) reported that in some case studies (for instance Wigley II at Fr=0.3 and Fr=0.4) it was not possible to stabilize the experiments, and therefore no results were obtained in those cases. This gives an idea on the complexity of carrying out this type of experiments, and the uncertainty that might be involved (Park et al. 2015). Moreover the added resistance in waves is a second-order force and usually quite small when compared to first-order forces, which makes very complicate to measure and separate both quantities. In fact, quite large models are needed to be able to measure second order forces, which is not the case of the referred experiments where the model length was 3 m. Since experimental data might have significant uncertainties, such results must be analyzed qualitatively rather than quantitatively.

Figure 10 shows a snapshot of the wave pattern generated by the Wigley III hull at Fr=0.2 advancing against a monochromatic wave with a wave length equal to the length of the hull. Figure 11 provides the time evolution of the resistance in still water and in wave for the same case. The added resistance can be obtained from the difference between the still water resistance and the mean value of the resistance in wave. Figure 12 shows the hull geometries and mesh sizes used.

Figure 13-16 show the heave and pitch RAOs, as well as the dimensionless added resistance ${\textstyle {R}_{aw}^{\ast }}$, versus the dimensionless wavelength for the four modified Wigley hull models.

Overall the results obtained with the FD-SLI and the FEM-SUPG schemes are quite similar to each other. Only in a few cases slight deviations are observed. Regarding the experimental results general trends are well captured, although in some cases some scattering is observed. Numerical results for RAOS and added resistance in waves follow reasonably well the experimental data although the goodness of the fitting depends on each case. Resonance frequencies are recovered well although peak values of added resistance are often underestimated.

Figure 10: Snapshot of wave pattern for Wigley I. Fr=0.2. λ_w/L=1.

Figure 11: Dimensionless time values of second-order-corrected longitudinal force for Wigley I. Fr=0.2. λ_w/L=1.

Figure 12: Mesh details and modified Wigley hulls view.

Figure 13: RAOs and ${\textstyle {\mathit {\boldsymbol {R}}}_{\mathit {\boldsymbol {aw}}}^{\mathit {\boldsymbol {\ast }}}}$for Wigley I hull.

Figure 14: RAOs and ${\textstyle {\mathit {\boldsymbol {R}}}_{\mathit {\boldsymbol {aw}}}^{\mathit {\boldsymbol {\ast }}}}$ for Wigley II hull.

Figure 15: RAOs and ${\textstyle {\mathit {\boldsymbol {R}}}_{\mathit {\boldsymbol {aw}}}^{\mathit {\boldsymbol {\ast }}}}$ for Wigley III hull.

Figure 16: RAOs and ${\textstyle {\mathit {\boldsymbol {R}}}_{\mathit {\boldsymbol {aw}}}^{\mathit {\boldsymbol {\ast }}}}$ for Wigley IV hull.

6. Summary and conclusion

A FEM based model to compute the wave making resistance in still water and added resistance in waves has been proposed. The proposed method solves the governing equations in the time-domain, using unstructured meshes, and is not constrained to linearized free surface boundary conditions. The mathematical model is based on potential and Stokes’ perturbation method, which makes it computationally attractive compared to CFD solvers. Two different numerical schemes have been proposed to solve the free surface boundary conditions: the first one is based on a third order FD-SLI scheme using three upwind plus one downwind points; and the second one is based on the FEM-SUPG stabilization.

The proposed schemes have been verified comparing against analytical solutions available for a moving pressure patch, and validated against experimental results by comparing wave making resistance and wave profiles. The verification and validation analyses have proved that fairly good results are obtained by the FD-SLI and FEM-SUPG schemes.

Regarding the use of linearized convective terms, the following conclusions are made: the NK linearization might be valid for low Froude numbers (lower than 0.15), but it is not advisable for higher velocities, even for slender bodies like the Wigley hull; wave making resistance predictions using the DB linearization are quite close to the NL approach.

The numerical results of added resistance in waves have been validated against experimental data available for four modified Wigley hulls at different Froude numbers and for a number of monochromatic waves. Added resistance highly depend on the wave induced heave and pitch movements, requiring a good calibration of the viscous damping is mandatory. The added resistance in waves is a second-order force and quite small when compared to first-order forces, which makes it very complicate to measure experimentally. In fact quite large models are needed to be able to measure second order forces, which is not the case of the refereed experiments where the model length was 3 m. Hence experimental data has significant uncertainties and its results must be analyzed qualitatively rather than quantitatively. Taking this into account, it can be concluded that the present methodology has been capable of estimating fairly well heave and pitch RAOs, and the added resistance trends.

Acknowledgements

This research work was partially supported by the X-SHEAKS project (ENE2014-59194-C2-1-R) of the Ministerio de Economía y Competitividad (Spain).

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