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**Ocean Science**
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**Research article**
13 Feb 2018

**Research article** | 13 Feb 2018

An analytical study of *M*_{2} tidal waves in the Taiwan Strait using an extended Taylor method

^{1}The First Institute of Oceanography, State Oceanic Administration, Qingdao, 266061, China^{2}Laboratory for Regional Oceanography and Numerical Modeling, Qingdao National Laboratory for Marine Science and Technology, Qingdao, 266237, China

^{1}The First Institute of Oceanography, State Oceanic Administration, Qingdao, 266061, China^{2}Laboratory for Regional Oceanography and Numerical Modeling, Qingdao National Laboratory for Marine Science and Technology, Qingdao, 266237, China

**Correspondence**: Guohong Fang (fanggh@fio.org.cn)

**Correspondence**: Guohong Fang (fanggh@fio.org.cn)

Abstract

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The tides in the Taiwan Strait (TS) feature large
semidiurnal lunar (*M*_{2}) amplitudes. An extended Taylor method is
employed in this study to provide an analytical model for the *M*_{2} tide
in the TS. The strait is idealized as a rectangular basin with a uniform
depth, and the Coriolis force and bottom friction are retained in the
governing equations. The observed tides at the northern and southern
openings are used as open boundary conditions. The obtained analytical
solution, which consists of a stronger southward propagating Kelvin wave, a
weaker northward propagating Kelvin wave, and two families of Poincaré
modes trapped at the northern and southern openings, agrees well with the
observations in the strait. The superposition of two Kelvin waves basically
represents the observed tidal pattern, including an anti-nodal band in the
central strait, and the cross-strait asymmetry (greater amplitudes in the
west and smaller in the east) of the anti-nodal band. Inclusion of
Poincaré modes further improves the model result in that the
cross-strait asymmetry can be better reproduced. To explore the formation
mechanism of the northward propagating wave in the TS, three experiments are
carried out, including the deep basin south of the strait. The results show
that the southward incident wave is reflected to form a northward wave by
the abruptly deepened topography south of the strait, but the reflected wave
is slightly weaker than the northward wave obtained from the above
analytical solution, in which the southern open boundary condition is
specified with observations. Inclusion of the forcing at the Luzon Strait
strengthens the northward Kelvin wave in the TS, and the forcing is thus of
some (but lesser) importance to the *M*_{2} tide in the TS.

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How to cite.

Wu, D., Fang, G., Cui, X., and Teng, F.: An analytical study of *M*_{2} tidal waves in the Taiwan Strait using an extended Taylor method, Ocean Sci., 14, 117–126, https://doi.org/10.5194/os-14-117-2018, 2018.

1 Introduction

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The Taiwan Strait (TS) is the sole passage connecting the East China Sea (ECS) and the South China Sea (SCS). The strait is approximately 350 km long, 200 km wide, and located mostly on the continental shelf with a mean depth of approximately 50 m. The bottom topography of the TS can be viewed as the extension of the ECS shelf in the north and becomes irregular in the south. The SCS deep basin is located south of the strait and is connected to the Pacific Ocean through the Luzon Strait (LS). An abrupt depth change is present between the TS and the SCS deep basin (Fig. 1).

The tides in the strait feature large *M*_{2} amplitudes. The greatest
amplitude, based on tidal gauge observations along the western Taiwan coast
reported by Jan et al. (2004b), is 1.73 m at Taichung and is 2.10 m at Matsu
near the mainland coast. Matsu is an island located approximately 20 km away
from the coast. Satellite observations indicate that the greatest amplitude
appears near Haitan Island (also called Pingtan Island),
located south of Matsu Island (also called Nangan Island; Fig. 2), and exceeds
2.2 m. Thus, the tidal regime of the *M*_{2} constituent has an anti-nodal band
near the cross-strait line from Haitan to Taichung, with greater amplitudes
in the west and smaller in the east, and this feature is called asymmetry by
Yu et al. (2015). Compared to *M*_{2}, which has a maximum amplitude over 2.2 m,
the amplitudes of the rest of the constituents are much smaller: the
maximum amplitudes of *S*_{2}, *K*_{1}, and *O*_{1} observed at 11 coastal
gauge stations reported by Jan et al. (2004b) are 0.66, 0.39, and 0.27 m,
respectively. Figure 2 displays the distribution of the *M*_{2} tidal
constituent based on the global tidal model DTU10, which is constructed on
the basis of multi-mission altimeter observations. Hereafter, we shall
regard the DTU10 model results as observations. The tides in the TS have
attracted a great number of studies since the 1980s. Yin and Chen (1982)
first developed a two-dimensional model for tides in the TS without showing
tidal currents. Fang et al. (1984) again developed a two-dimensional model
and obtained a rather accurate distribution of tidal currents. They suggested
that the semidiurnal tidal motion in the TS was maintained mainly by the
energy flux from the ECS and partly by that from the SCS. Ye et al. (1985)
and Lü and Sha (1999) developed three-dimensional models for the strait
and also found that the southward energy flux of semidiurnal tides from the
ECS was much greater than the northward flux. Lin et al. (2000, 2001)
emphasized the anomalous amplification of semidiurnal tides in the strait,
and attributed the amplification to a resonance. Jan et al. (2004b) modelled
the tides using an optimization approach. Zhu et al. (2009), Hu et al. (2010), and
Zeng et al. (2012) further developed more accurate numerical
models. Yu et al. (2017) studied the propagation and dissipation of tidal
waves in the strait. It has been well recognized from these numerical
investigations that the semidiurnal tides in the TS consist mainly of two
oppositely propagating waves, one from north to south and another from south
to north. In particular, Fang et al. (1984, 1999) and Ye et al. (1985)
suggested that the semidiurnal tidal motion in the TS was maintained mainly
by the energy flux from the ECS and partly by that from the SCS. Jan et al. (2002, 2004a)
further noticed that the southward propagating wave could be
reflected when encountering the sharply deepened bottom topography south of
the strait and suggested that the reflected wave is the main component of
the northward propagating wave and that the contribution of the SCS is
negligible. Yu et al. (2015) completed an extensive numerical study of the
formation of the *M*_{2} tide in the strait with a special focus on the
asymmetric nature in the cross-strait direction.

The existing studies almost all employed data analysis and numerical modelling, except that some simple dynamical analyses were performed using one-dimensional solutions to explain the model results by Jan et al. (2002) and Yu et al. (2015). The purpose of the present study is to establish two-dimensional analytical models using an extended Taylor method (see Sect. 2 for details). In the analytical models, the classical Kelvin waves and Poincaré modes in idealized basins are used to approximately represent the tides in the natural basin. This enables us to estimate the strengths of the southward and the northward waves to reveal the role of each classical wave in the formation of the tides in the strait and to clarify how the waves are generated. In particular, we can roughly estimate the relative importance of the reflected wave at the steep topography versus the incident wave from the LS in the formation of the northward Kelvin wave in the TS.

The Taylor problem is a classical tidal dynamic problem (Hendershott and
Speranza, 1971). Since his pioneering work, Taylor's method has been
subsequently developed and applied to many sea areas (e.g. Table 1 of Roos
et al., 2011). In the previous applications, most of the studied basins have
a closed end that can almost perfectly reflect the incident tidal wave, thus
closely retaining the phase of the tidal elevation. In contrast, the
topographic step south of the TS acts as a permeable interface that can only
partially reflect the incident wave, and furthermore, the elevation phase of
the reflected wave is changed by nearly 180^{∘} at the step (see
Sect. 5.5 of Dean and Dalrymple, 1984). Therefore, the strait is also a
locality of particular interest for the application of Taylor's method.

2 Model formulation and solution method

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Taylor (1922) first presented an analytical solution for tides in a semi-infinite rotating rectangular channel of uniform depth to explain the existence of amphidromic systems in gulfs. His solution showed that the tide in such a channel can be represented by the superposition of an incident Kelvin wave, a reflected Kelvin wave, and a family of Poincaré modes trapped near the closed end. In 1925, Defant simplified Taylor's solution approach by applying the collocation method (see Defant, 1961, pp. 213–215). In the original version of Taylor's problem, as well as Defant's approach, the friction and open boundary condition were left out of consideration. Fang and Wang (1966) and Rienecker and Teubner (1980) extended the Taylor problem by taking friction into consideration in the governing equations. The introduction of friction can explain why the amphidromic point in the Northern Hemisphere shifts from the central axis toward the right, as seen from the closed end and looking seaward. The mechanism of the shift of the amphidromic point was also explained by Hendershott and Speranza (1971), in which the dissipation was assumed to occur at the closed end of the basin rather than during the wave propagation. Fang et al. (1991) further extended the Taylor problem by introducing the open boundary condition, enabling solutions accounting for the finite length of the basin. Jung et al. (2005), Roos and Schuttelaars (2011), and Roos et al. (2011) further extended the Taylor method to model tides in multiple rectangular basins. The solution method used in the present study is basically the same as Fang et al. (1991), but with minor correction and generalization, as was done in studies of Jung et al. (2005), Roos and Schuttelaars (2011), and Roos et al. (2011). The analytical method initiated by Taylor and developed afterward is called an extended Taylor method in this paper.

The governing equations used in this study are as follows:

$$\begin{array}{}\text{(1)}& {\displaystyle}\left\{\begin{array}{l}{\displaystyle \frac{\partial \stackrel{\mathrm{\u0303}}{u}}{\partial t}}-f\stackrel{\mathrm{\u0303}}{v}=-g{\displaystyle \frac{\partial \stackrel{\mathrm{\u0303}}{\mathit{\zeta}}}{\partial x}}-\mathit{\gamma}\stackrel{\mathrm{\u0303}}{u},\\ {\displaystyle \frac{\partial \stackrel{\mathrm{\u0303}}{v}}{\partial t}}+f\stackrel{\mathrm{\u0303}}{u}=-g{\displaystyle \frac{\partial \stackrel{\mathrm{\u0303}}{\mathit{\zeta}}}{\partial y}}-\mathit{\gamma}\stackrel{\mathrm{\u0303}}{v},\\ {\displaystyle \frac{\partial \stackrel{\mathrm{\u0303}}{\mathit{\zeta}}}{\partial t}}=-h\left[{\displaystyle \frac{\partial \stackrel{\mathrm{\u0303}}{u}}{\partial x}}+{\displaystyle \frac{\partial \stackrel{\mathrm{\u0303}}{v}}{\partial y}}\right],\end{array}\right.\end{array}$$

where *t* represents time; (*x*,*y*) are the Cartesian
coordinates; ($\stackrel{\mathrm{\u0303}}{u},\stackrel{\mathrm{\u0303}}{v}$) are the
depth-averaged velocity components in the (*x*,*y*)
directions, respectively; $\stackrel{\mathrm{\u0303}}{\mathit{\zeta}}$ is the tidal elevation; *h* is the water depth,
assumed uniform; *γ* is the frictional coefficient, taken as a
constant; *g*=9.8 ms^{−2} is the acceleration due to gravity;
and *f* is the Coriolis parameter, also taken as a constant due to the
smallness of the study area. The set of equations in Eq. (1) are two-dimensional
linearized shallow water equations on an *f* plane with the momentum
advection neglected. The equations are the same as those used in the work of
Taylor (1922), except that the bottom friction is incorporated, as in Fang
and Wang (1966) and Rienecker and Teubner (1980). When a monochromatic wave
is considered, $\left(\stackrel{\mathrm{\u0303}}{\mathit{\zeta}},\stackrel{\mathrm{\u0303}}{u},\stackrel{\mathrm{\u0303}}{v}\right)$
can be expressed as follows:

$$\begin{array}{}\text{(2)}& {\displaystyle}\left(\stackrel{\mathrm{\u0303}}{\mathit{\zeta}},\stackrel{\mathrm{\u0303}}{u},\stackrel{\mathrm{\u0303}}{v}\right)=Re\left\{\left(\mathit{\zeta},u,v\right){e}^{i\mathit{\sigma}t}\right\},\end{array}$$

where $\left(\mathit{\zeta},u,v\right)$ are complex amplitudes
of $\left(\stackrel{\mathrm{\u0303}}{\mathit{\zeta}},\stackrel{\mathrm{\u0303}}{u},\stackrel{\mathrm{\u0303}}{v}\right)$,
respectively, *σ* is the angular frequency of the wave, and
$i\equiv \sqrt{-\mathrm{1}}$. For this wave, the set of equations in Eq. (1)
reduce as follows:

$$\begin{array}{}\text{(3)}& {\displaystyle}\left\{\begin{array}{l}\left(\mathit{\mu}+i\right)u-\mathit{\nu}v=-{\displaystyle \frac{g}{\mathit{\sigma}}}{\displaystyle \frac{\partial \mathit{\zeta}}{\partial x}},\\ \left(\mathit{\mu}+i\right)v+\mathit{\nu}u=-{\displaystyle \frac{g}{\mathit{\sigma}}}{\displaystyle \frac{\partial \mathit{\zeta}}{\partial y}},\\ \mathit{\zeta}={\displaystyle \frac{ih}{\mathit{\sigma}}}\left[{\displaystyle \frac{\partial u}{\partial x}}+{\displaystyle \frac{\partial v}{\partial y}}\right],\end{array}\right.\end{array}$$

in which $\mathit{\mu}=\frac{\mathit{\gamma}}{\mathit{\sigma}}$ and $\mathit{\nu}=\frac{f}{\mathit{\sigma}}$.

Considering a rectangular basin with two parallel sidewalls of length *L*
and with a width *B*, we placed the *x* axis along a sidewall and the *y*
axis perpendicular to the *x* axis and pointing to the other sidewall. Thus,
the basin is confined by $x=\mathrm{0},L$ and $y=\mathrm{0},B$,
respectively. The boundary conditions along the sidewalls are taken as
follows:

$$\begin{array}{}\text{(4)}& {\displaystyle}v=\mathrm{0}\phantom{\rule{0.25em}{0ex}}\text{at}\phantom{\rule{0.25em}{0ex}}y=\mathrm{0}\phantom{\rule{0.25em}{0ex}}\text{and}\phantom{\rule{0.25em}{0ex}}y=B\end{array}$$

within $x\in (\mathrm{0},L)$. Along the cross sections,
*x*=0 and *x*=*L*, various choices of boundary conditions
are applicable depending on the problem concerned:

$$\begin{array}{}\text{(5)}& {\displaystyle}u=\mathrm{0}\end{array}$$

if the cross section is a closed boundary;

$$\begin{array}{}\text{(6)}& {\displaystyle}u=\pm \sqrt{{\displaystyle \frac{g}{(\mathrm{1}-i\mathit{\mu})h}}}\mathit{\zeta}\end{array}$$

if the free radiation in the positive/negative *x* direction occurs on the cross section;

$$\begin{array}{}\text{(7)}& {\displaystyle}\mathit{\zeta}=\widehat{\mathit{\zeta}}\end{array}$$

if the tidal elevation is specified as $\widehat{\mathit{\zeta}}$
along the cross section;

and/or

$$\begin{array}{}\text{(8)}& {\displaystyle}{\mathit{\zeta}}_{\mathrm{A}}={\mathit{\zeta}}_{\mathrm{B}}\phantom{\rule{0.25em}{0ex}}\text{and}\phantom{\rule{0.25em}{0ex}}{u}_{\mathrm{A}}{h}_{\mathrm{A}}={u}_{\mathrm{B}}{h}_{\mathrm{B}}\end{array}$$

if the cross section is a connecting boundary of two basins A
and B, each with a different uniform depth of *h*_{A} and *h*_{B}.

Eq. (8) show the matching conditions accounting for sea level
continuity and volume transport continuity, respectively. The individual
conditions in Eqs. (5) to (8), or their combination, may be used as boundary
conditions at the cross sections *y*=0 and *B*. The relationship between *u* and *ζ*
shown in Eq. (6) is based on the solution for progressive Kelvin waves in the
presence of friction, which will be given in Eqs. (9) and (10) below. If
*μ* ≪ 1, a simpler equation, $u=\pm \sqrt{\frac{g}{h}}\mathit{\zeta}$, can be used to replace Eq. (6).

The governing set of equations in Eq. (3) have only the following four forms satisfying
the sidewall boundary condition of Eq. (4) (see Fang et al., 1991; an error in
the equation for *β* in their paper has been corrected here. Note that the
error occurred during the preparation of their manuscript and the correct
expression was used in their computations):

$$\begin{array}{}\text{(9)}& \left\{\begin{array}{l}{v}_{\mathrm{1}}=\mathrm{0}\phantom{\rule{0.125em}{0ex}},\\ {u}_{\mathrm{1}}=-a\phantom{\rule{0.125em}{0ex}}\mathrm{exp}\left(\mathit{\alpha}y+i\mathit{\beta}x\right),\\ {\mathit{\zeta}}_{\mathrm{1}}={\displaystyle \frac{\mathit{\beta}}{\mathit{\sigma}}}ha\mathrm{exp}\left(\mathit{\alpha}y+i\mathit{\beta}x\right),\end{array}\right.\end{array}$$

$$\begin{array}{}\text{(10)}& \left\{\begin{array}{l}{v}_{\mathrm{2}}=\mathrm{0},\\ {u}_{\mathrm{2}}=b\phantom{\rule{0.125em}{0ex}}\mathrm{exp}\left[-\left(\mathit{\alpha}y+i\mathit{\beta}x\right)\right],\\ {\mathit{\zeta}}_{\mathrm{2}}={\displaystyle \frac{\mathit{\beta}}{\mathit{\sigma}}}hb\phantom{\rule{0.125em}{0ex}}\mathrm{exp}\left[-\left(\mathit{\alpha}y+i\mathit{\beta}x\right)\right],\end{array}\right.\end{array}$$

$$\begin{array}{}\text{(11)}& \left\{\begin{array}{l}{v}_{\mathrm{3}}=\sum _{n=\mathrm{1}}^{\mathrm{\infty}}{\mathit{\kappa}}_{n}\mathrm{sin}{r}_{n}y\mathrm{exp}\left(-{s}_{n}x\right),\\ {u}_{\mathrm{3}}=\sum _{n=\mathrm{1}}^{\mathrm{\infty}}{\mathit{\kappa}}_{n}\left({A}_{n}\mathrm{cos}{r}_{n}y+{B}_{n}\mathrm{sin}{r}_{n}y\right)\mathrm{exp}\left(-{s}_{n}x\right),\\ {\mathit{\zeta}}_{\mathrm{3}}={\displaystyle \frac{ih}{\mathit{\sigma}}}\sum _{n=\mathrm{1}}^{\mathrm{\infty}}{\mathit{\kappa}}_{n}\left({C}_{n}\mathrm{cos}{r}_{n}y+{D}_{n}\mathrm{sin}{r}_{n}y\right)\mathrm{exp}\left(-{s}_{n}x\right),\end{array}\right.\end{array}$$

and

$$\begin{array}{}\text{(12)}& \left\{\begin{array}{l}{v}_{\mathrm{4}}=\sum _{n=\mathrm{1}}^{\mathrm{\infty}}{\mathit{\lambda}}_{n}\mathrm{sin}{r}_{n}y\mathrm{exp}\left[-{s}_{n}\left(L-x\right)\right],\\ {u}_{\mathrm{4}}=\sum _{n=\mathrm{1}}^{\mathrm{\infty}}{\mathit{\lambda}}_{n}\left({A}_{n}^{\prime}\mathrm{cos}{r}_{n}y+{B}_{n}^{\prime}\mathrm{sin}{r}_{n}y\right)\mathrm{exp}\left[-{s}_{n}\left(L-x\right)\right],\\ {\mathit{\zeta}}_{\mathrm{4}}={\displaystyle \frac{ih}{\mathit{\sigma}}}\sum _{n=\mathrm{1}}^{\mathrm{\infty}}{\mathit{\lambda}}_{n}\left({C}_{n}^{\prime}\mathrm{cos}{r}_{n}y+{D}_{n}^{\prime}\mathrm{sin}{r}_{n}y\right)\mathrm{exp}\left[-{s}_{n}\left(L-x\right)\right],\end{array}\right.\end{array}$$

where

$$\begin{array}{}\text{(13)}& {\displaystyle}& {\displaystyle}\mathit{\alpha}={\displaystyle \frac{\mathit{\nu}}{{\left(\mathrm{1}-i\mathit{\mu}\right)}^{\frac{\mathrm{1}}{\mathrm{2}}}}}k,\text{(14)}& {\displaystyle}& {\displaystyle}\mathit{\beta}={\left(\mathrm{1}-i\mathit{\mu}\phantom{\rule{0.125em}{0ex}}\right)}^{\frac{\mathrm{1}}{\mathrm{2}}}k,\text{(15)}& {\displaystyle}& {\displaystyle}{r}_{n}={\displaystyle \frac{n\mathit{\pi}}{B}},\text{(16)}& {\displaystyle}& {\displaystyle}{s}_{n}={\left({r}_{n}^{\mathrm{2}}+{\mathit{\alpha}}^{\mathrm{2}}-{\mathit{\beta}}^{\mathrm{2}}\right)}^{\frac{\mathrm{1}}{\mathrm{2}}},\end{array}$$

in which $k=\mathit{\sigma}/\phantom{\mathit{\sigma}c}c$ is the wave number, with $c=\sqrt{gh}$ being the wave speed of the Kelvin wave in the absence of friction.
In Eq. (16), *s*_{n} has two complex values for each *n*, and here, we
choose the one that has a positive real part. To satisfy equations in Eq. (3),
(${A}_{n},{B}_{n},{C}_{n},{D}_{n})$ and
$({A}_{n}^{\prime},{B}_{n}^{\prime},{C}_{n}^{\prime},{D}_{n}^{\prime})$ should be as follows:

$$\begin{array}{}\text{(17)}& {\displaystyle}& {\displaystyle}{A}_{n}={\displaystyle \frac{\left[{\left(\mathit{\mu}+i\right)}^{\mathrm{2}}+{\mathit{\nu}}^{\mathrm{2}}\right]{r}_{n}{s}_{n}}{{\left(\mathit{\mu}+i\right)}^{\mathrm{2}}{r}_{n}^{\mathrm{2}}+{\mathit{\nu}}^{\mathrm{2}}{s}_{n}^{\mathrm{2}}}},\text{(18)}& {\displaystyle}& {\displaystyle}{B}_{n}={\displaystyle \frac{\mathit{\nu}\left(\mathit{\mu}+i\right)\left({\mathit{\alpha}}^{\mathrm{2}}-{\mathit{\beta}}^{\mathrm{2}}\right)}{{\left(\mathit{\mu}+i\right)}^{\mathrm{2}}{r}_{n}^{\mathrm{2}}+{\mathit{\nu}}^{\mathrm{2}}{s}_{n}^{\mathrm{2}}}},\text{(19)}& {\displaystyle}& {\displaystyle}{C}_{n}={r}_{n}-{s}_{n}{A}_{n},\text{(20)}& {\displaystyle}& {\displaystyle}{D}_{n}=-{s}_{n}{B}_{n},\text{(21)}& {\displaystyle}& {\displaystyle}{A}_{n}^{\prime}=-{A}_{n},\text{(22)}& {\displaystyle}& {\displaystyle}{B}_{n}^{\prime}={B}_{n},\text{(23)}& {\displaystyle}& {\displaystyle}{C}_{n}^{\prime}={C}_{n},\text{(24)}& {\displaystyle}& {\displaystyle}{D}_{n}^{\prime}=-{D}_{n}.\end{array}$$

Equations (9) and (10) represent Kelvin waves propagating in the −*x*
and *x* directions, respectively; Eqs. (11) and (12) represent two families
of Poincaré modes trapped at the cross sections *x*=0, *L*,
respectively. Coefficients $(a,b,{\mathit{\kappa}}_{n},{\mathit{\lambda}}_{n})$ are
related to amplitudes and phases of Kelvin waves and Poincaré modes.
These coefficients are to be determined by boundary conditions.

The collocation method is convenient when determining the coefficients
$(a,b,{\mathit{\kappa}}_{n},{\mathit{\lambda}}_{n})$. The calculation procedure can be as
follows. First, we truncate the family of Poincaré modes, Eqs. (11) and
(12), at the *N*th order, so that the number of undetermined coefficients for
Poincaré modes is 2*N* and the total number of undetermined
coefficients (plus those for Kelvin waves) is thus 2*N*+2. To
determine these unknowns, we take equally spaced *N*+1 dots, called
collocation points, located at $y=\frac{B}{\mathrm{2}(N+\mathrm{1})},\frac{\mathrm{3}B}{\mathrm{2}(N+\mathrm{1})},\mathrm{\dots},\frac{\left(\mathrm{2}N+\mathrm{1}\right)B}{\mathrm{2}(N+\mathrm{1})}$ on
both cross sections *x*=0 and *L*. At these points, one of the
boundary conditions given by Eqs. (5)–(8) should be satisfied. This yields
2*N*+2 equations. By solving this system of equations, we can
obtain 2*N*+2 coefficients $(a,b,{\mathit{\kappa}}_{n},{\mathit{\lambda}}_{n})$.
Since the high-order Poincaré modes decay from the boundary very quickly
as can be seen from large *s*_{n} in Eqs. (11) and (12), it is generally
necessary to retain only a few lower order terms.

3 Application to the Taiwan Strait

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In this section, we will first establish an idealized analytical model for
the TS. The strait is idealized as a rectangular basin with two sidewalls
roughly along the China mainland and Taiwan coastlines (as shown in Fig. 1).
The width and length of the model domain are taken as *B*=200 km and
*L*=330 km, respectively. The depth is taken as *h*=52 m, a mean depth
calculated based on ETOPO1. We place the origin of the coordinates at the
northernmost corner of the rectangle, the *x* axis along the mainland coast,
and the *y* axis in an offshore direction. The axis of the strait is toward
the south to southwest. However, to keep it short, we will hereafter simply
use “south” to refer to “south to southwest”, and similarly for other
directions. The Coriolis parameter *f* is taken as $\mathrm{0.594}\times {\mathrm{10}}^{-\mathrm{4}}$ s^{−1},
corresponding to a latitude of $\mathit{\phi}=\mathrm{24}{}^{\circ}$ N. The angular frequency of the *M*_{2} tide
is $\mathrm{1.4052}\times {\mathrm{10}}^{-\mathrm{4}}$ s^{−1}. The
friction coefficient *γ* can be estimated from the relation $\mathit{\gamma}={C}_{\mathrm{D}}\left(\frac{\mathrm{8}}{\mathrm{3}\mathit{\pi}}\right)\frac{U}{h}$,
in which *C*_{D}
and *U* represent the drag coefficient and amplitude of the *M*_{2} tidal
current, respectively (e.g. Chapter 8 of Dronkers, 1964). In this study, we
take *C*_{D}=0.0026 and *U*=0.5 m s^{−1} based on the numerical results of Fang
et al. (1984), and then $\mathit{\mu}=\mathit{\gamma}/\mathit{\sigma}$ is
approximately equal to 0.15. From these parameter values, we can obtain the
wavelength of the *M*_{2} Kelvin wave as 1009 km. Since the basin width is
smaller than half of the Kelvin wavelength, the Poincaré modes can only
exist in a bound form (Godin, 1965; Fang and Wang, 1966). The e-folding
length of decay of the lowest Poincaré mode is approximately 63 km; that
is, the amplitude of this mode reduces to approximately 37 % relative to
its maximum value at a distance of 63 km away from the boundary.
Equivalently, it may also reduce to approximately 20 % relative to its
maximum value at a distance of 100 km. The length scales of decay for higher
order Poincaré modes are even shorter.

In this study, the families of Poincaré modes are truncated at *N*=19
and 20 collocation points set along both the northern and southern open
boundaries. The boundary condition (Eq. 7) is employed with the values of
$\widehat{\mathit{\zeta}}$ equal to the observed harmonic constants from the global tide
model DTU10 (Cheng and Anderson, 2011).

The obtained analytical solution of the *M*_{2} constituents is shown in
Fig. 3a. For comparison, the observed *M*_{2} tidal system chart based on
DTU10 is also shown in Fig. 3b. Although the complicated bottom topography
and the irregular coastlines are greatly simplified, the analytical model
still agrees well with the observation. The observed tidal regime features
significantly greater amplitudes along the mainland coast than along the
Taiwan coast, showing the cross-strait asymmetry. The phase-lags near the
mainland coast increase from north to south, showing a progressive wave
nature, while those near the middle Taiwan coast have only small changes,
showing a standing wave nature. That is, along the Taiwan coast the wave
propagates southward in the northern area and propagates northward in the
southern area. The largest amplitudes are roughly along the cross section of
150 km and appears as an anti-nodal band. The phase-lags in this band range
from 80 to 90^{∘}. These features have all been
reproduced in the analytical model.

To reveal the relative importance of the Kelvin waves and Poincaré modes in the model, the superposition of two Kelvin waves is given in Fig. 3c and that of the Poincaré modes is given in Fig. 3d. The contribution of the Poincaré modes is observed to be much smaller than that of the Kelvin waves. The tidal system chart constructed using only superposed Kelvin waves (Fig. 3c) resembles the complete model (Fig. 3a) and the observation (Fig. 3b) quite well, though the inclusion of the Poincaré modes improves the model to a certain degree. From Fig. 3a we can see that the difference between the highest amplitude on the west sidewall and that on the east sidewall in the anti-nodal band is approximately 0.4 m, while the corresponding difference shown in Fig. 3c is approximately 0.2 m. Thus, approximately half of the cross-strait asymmetry is explained by the superposition of two oppositely propagating Kelvin waves, with the southward one being stronger than the one moving northward. Here, both the Coriolis force and the weaker northward wave are the major factors. The superposition of Poincaré modes in this band has an amplitude of approximately 0.1 m on both sides and has nearly the same phase-lag as the superposed Kelvin wave on the west and a nearly opposite phase-lag to the superposed Kelvin wave on the east. Therefore, the superposed Poincaré modes play a role to increase the amplitudes in the west and reduce the amplitudes in the east and hence enhances the asymmetry. The superposed Poincaré modes make nearly the same contribution to the cross-strait asymmetry as the superposed Kelvin wave.

From the comparison, we find that the amplitude variation along the northern
boundary in Fig. 3c is less than that in Fig. 3a. This shows that near the
boundary, the Poincaré modes are of a certain importance. The existence
of the Poincaré modes is related to the fact that the *M*_{2} tide is
from the Pacific Ocean; its amplitude increases from the deeper outer shelf
toward the shallower inner shelf. This amplitude variation cannot be
completely represented by the superposed Kelvin wave at a uniform depth, and
superposed Poincaré modes are necessary to compensate for their
difference. The situation at the southern boundary is similar. The
distribution of the superposed Poincaré modes in the anti-nodal band is
clearly related to those at the northern and southern openings (Fig. 3d). Yu
et al. (2015) suggested that the orientation of the topographic step south
of the strait was not perpendicular to the strait axis but has an angle.
This might cause the reflected wave to propagate toward the mainland coast
and thus amplify the tides there. The present solution indicates that the
obliqueness of the topographic step south of the TS may also play a role in
the formation of the cross-strait asymmetry, as suggested by Yu et al. (2015), but it seems not to be a controlling factor.

The obtained analytical solution enables us to see the magnitudes and
characteristics of both the southward and northward Kelvin waves. These two
oppositely propagating waves, which correspond to Eqs. (9) and (10),
respectively, are displayed separately in Fig. 4a and b. From Fig. 4a, we
see that the phase-lag of the southward wave increases from north to south.
The amplitude deceases from north to south due to friction and from west to
east due to the Coriolis effect. The characteristics of the northward wave
are the opposite. The area mean amplitude of the southward wave is 1.18 m,
while that of the northward wave is 0.84 m, smaller than the former by
0.34 m. Along the western sidewall, the amplitudes of the southward wave range
from approximately 1.4 to 1.6 m, while those of the northward wave range
from approximately 0.6 to 0.7 m; thus, the superposition of the waves is
dominated by the former and appears as a southward progressive wave. Around
the cross section *x*≈150 km, the phase-lags of the
southward and northward waves are nearly equal, between 80 and
90^{∘}. Thus, the superposed tides here have the greatest amplitudes
equal to the sum of the amplitudes of these two waves, exceeding 2.1 m, as
already seen in Fig. 3c. Along the eastern sidewall, however, the
differences in amplitudes of the southward and northward waves are much
smaller, and thus the superposition of the waves tends to appear as a
standing wave. Around the point *x*≈150 km, the phase-lags
of the southward and northward waves are also nearly equal. Thus, the
amplitude of the combined tide is also relatively large, equal to the sum of
the amplitudes of these two waves; but now it is only slightly greater than
1.9 m, which is smaller than the corresponding value at the western
sidewall.

4 Formation mechanism of the northward Kelvin wave in the Taiwan Strait

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In the preceding section, we have shown that the northward Kelvin wave is weaker than the southward wave on average, but they have a similar magnitude along the Taiwan coast. In this section, we will examine the formation mechanism of the northward Kelvin wave. There are two possible origins for the northward Kelvin wave in the TS. One is the reflection of the southward wave at the sharply deepened topography and another is an incident wave from the LS propagating toward the TS. In the following, we examine their respective contributions by using the extended Taylor models.

Three experiments have been carried out to explore the formation mechanism
of the northward Kelvin wave in the TS. The first experiment (denoted as Ex. 1)
has the model geometry shown in Fig. 5a. The TS is represented by area A,
with the width and depth equal to the above single area model. Since the
topographic step is located away from the southern boundary of the single
area model domain (Fig. 1), we extend the length of the area to 400 km. Area
B represents the deep basin south of the topographic step, and the water
depth of the deep basin is taken as 1000 m, as was done in Jan et al. (2002, 2004). The purpose of this experiment is to examine the effect of the
topographic step in reflecting the incident wave from the ECS. The
experimental design for area A is similar to that of Roos and Schuttelaars (2011): a southward Kelvin wave is specified to be identical to the single
basin solution, as shown in Fig. 4a in the preceding section. The
Poincaré modes trapped at the cross section *x*=0 are
neglected, while those trapped at the cross section *x*=400 km are
retained. The matching condition (Eq. 8) is applied at the connecting boundary
of areas A and B, and the radiative condition (Eq. 6) is used at the
southernmost opening.

Figure 5b displays the solution of Ex. 1. It can be seen that the basic
pattern of the tidal regime is similar to that of the single area model
solution shown in Fig. 3c. In particular, there is again an anti-nodal band
near *x*=150 km, though the amplitudes in this band produced by
this experiment are smaller than those given in Fig. 3c. The smallest
amplitudes appear along the connecting cross section, showing that a nodal
band exists there. Therefore, the anti-node is located approximately 250 km
away from the topographic step. The wavelength of the *M*_{2} tide in a
channel of a uniform depth of 52 m is equal to 1009 km, and so the distance
between the anti-node and the topographic step is equal to one-quarter of
the wavelength. This result further implies that if the channel were 500 km long,
resonance would occur. However, Taiwan Island is approximately 380 km long and is
not able to support a resonance for the *M*_{2} constituent. In
fact, the resonant period of the TS is 13.5 h, according to the experiments
performed by Cui et al. (2015), which is almost the same as one of the
resonant periods of the ECS (13.7 h, obtained by Cui et al., 2015). This
means that the tidal response in the TS is not independent, but rather
closely related to the tides in the ECS.

The southward and northward Kelvin waves obtained from Ex. 1 are shown in
Figs. 5c and d, respectively. Comparison of these figures with Figs. 4a and
b indicates that in area A, the southward wave is identical, but the
northward wave from Ex. 1 is weaker. For the area *x*=0 to 330 km and *y*=0
to 200 km, the area mean amplitude of the northward
Kelvin wave is 0.57 m, which is smaller than the single area model value by
32 %. In area B, the amplitudes of the transmitted southward Kelvin wave
are approximately 0.4 m, and those of the northward wave are negligible. An
important difference in the co-phase-lag distributions is that Figs. 3a–c
show a northward propagation along the southern part of the eastern
sidewall, while Fig. 5b does not have such a feature. This is because in the
single area case, the amplitudes of the northward Kelvin wave are greater
than those of the southward Kelvin wave in this area (Fig. 4a, b), while
in Ex. 1, this situation does not occur (Fig. 5c, d).

The relative magnitudes of the incident and the reflected and transmitted
Kelvin waves can be evaluated by comparing their amplitudes along the
connecting cross section at *x*=400 km. The sectional mean
amplitudes for the incident, reflected, and transmitted waves,
*H*_{i}, *H*_{r}, and *H*_{t}, are 1.06, 0.64, and
0.40 m, respectively (Figs. 5c, d). Thus, the ratios *H*_{r}∕*H*_{i}
and *H*_{t}∕*H*_{i} are equal to 0.61 and 0.37,
respectively. The corresponding values based on the theory ignoring the
earth's rotation can be calculated from
$\frac{{H}_{\mathrm{r}}}{{H}_{\mathrm{i}}}=\frac{\mathrm{1}-\mathit{\rho}}{\mathrm{1}+\mathit{\rho}}$ and
$\frac{{H}_{\mathrm{t}}}{{H}_{\mathrm{i}}}=\frac{\mathrm{2}\mathit{\rho}}{\mathrm{1}+\mathit{\rho}}$ with $\mathit{\rho}=\sqrt{{h}_{\mathrm{A}}/{h}_{\mathrm{B}}}$ (e.g. Dean and Dalrymple, 1984, p. 144).
Substitution of the present model depths into these equations yields
${H}_{\mathrm{r}}/{H}_{\mathrm{i}}=\mathrm{0.63}$ and
${H}_{\mathrm{t}}/{H}_{\mathrm{i}}=\mathrm{0.37}$. This indicates that
the magnitude of the reflected waves in the two-dimensional case with the
earth's rotation being taken into account is smaller than that based on the
theory with the earth's rotation being ignored.

From Fig. 1, we can see that there is a narrow shelf along the mainland coast. To simulate the effect of the narrow shelf on the tides in the TS, we performed a second experiment, numbered Ex. 2. In this experiment, the deep basin has moved 60 km eastward, allowing the tides in the shallow basin to freely radiate southward as shown in Fig. 6a. The radiative condition (Eq. 6) is retained along the southernmost opening. The results of Ex. 2 are given in Fig. 6. It can be seen that the tides in area A have only small changes, though the deep basin has moved 60 km eastward. Observable changes can only be found in area B where the tidal amplitudes are slightly reduced.

The purpose of performing a third experiment, numbered Ex. 3, is to consider
the tidal input from the LS. The major difficultly in including the LS input
in Taylor's model for the TS is that the LS has a meridional orientation,
while Taylor's model does not allow any part of the sidewalls to open. Here,
we will use a rather crude model to solve this issue. We use the same model
domain as Ex. 2, but the radiative boundary condition (Eq. 6) is retained only
for the west segment of the southernmost opening, and the boundary condition
(Eq. 7) is applied to the remaining east segment of the opening. From Fig. 1, we
can see that the cross section from the mainland shelf to the LS is much
longer than the width of the LS. Thus, in our model, we take the lengths of
the west and east segments to be 120 and 80 km, respectively, as shown in
Fig. 7a. In addition, from Fig. 2, we observe that the tidal amplitude along
the LS is roughly 0.2 m, and the phase-lag is approximately 310^{∘}.
Since a significant portion of the incident wave from the LS propagates
toward the SCS deep basin (e.g. Fang et al., 1999; Yu et al., 2015), we
use a 0.1 m amplitude and 310^{∘} phase-lag as an open boundary
condition for the east segment of the southernmost opening in Ex. 3. The
model results are given in Fig. 7b to d. From Fig. 7b, we can see that the
amplitudes of the tide in area A now become greater than the results of Ex. 2 (Fig. 6b),
and a northward propagating character can be seen in the
south-eastern portion of area A. These improvements can be attributed to the
increased amplitudes of the northward Kelvin wave (Figs. 6d, 7d).

5 Summary and discussion

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In the present study, we first established an analytical model for the
*M*_{2} tide in the TS using the extended Taylor method. The superiority of
the analytical solution is that the tides can be decomposed into a southward
Kelvin wave, a northward Kelvin wave, and two families of Poincaré
modes, providing a deeper insight into the dynamics of the tides in the
area. Though the coastlines and bottom topography are greatly simplified,
the model-produced pattern resembles the observed tidal regime quite well.
We then carried out several experiments to examine the formation mechanism
of the northward propagating wave, especially the roles of the abruptly
deepened bottom topography south of the TS and the tidal forcing in the LS
in the formation of the northward wave. From this study, we have obtained
the following results.

The *M*_{2} tide in the TS can be basically represented by the superposition
of a southward propagating and a northward propagating Kelvin wave, with the
former being stronger than the latter. The superposed Kelvin waves give an
anti-nodal band near the cross-strait transection, roughly from Haitan
Island to Taichung. The maximum amplitude on the mainland side is greater
than that on the Taiwan side, showing the cross-strait asymmetry. Therefore,
the observed features can be reproduced by the superposition of a stronger
southward propagating and a weaker northward propagating Kelvin wave. In
this regard, the Coriolis force and the weaker northward wave play essential
roles.

Inclusion of the Poincaré modes in the analytical model improves the model results: the east to west increase in amplitudes along the northern and southern openings is better reproduced; and in particular, the Poincaré modes make approximately the same contribution as the Kelvin waves to the cross-strait asymmetry in the anti-nodal band.

The reflection of the southward wave at the abruptly deepened topography
south of the TS is a major contribution to the formation of the northward
propagating wave in the strait. However, the reflected wave is slightly
weaker than that obtained from the analytical solution with open boundary
conditions determined by the observations. Inclusion of the tidal forcing at
the LS strengthens the northward Kelvin wave in the TS and thus improves the
model result. This indicates that the LS forcing is of some (but lesser)
importance to the *M*_{2} tide in the TS.

The analytical solutions can help us to understand the dynamics of tidal motion in the TS, but there are some limitations. For example, the LS is located on the east side of the study area, while the Taylor model does not allow for a forcing on the sidewalls, and thus we are bound to let a part of southern opening represent the LS (Fig. 7a). In addition, we have assumed that the water depth changes from 52 to 1000 m immediately at the connecting cross section without considering the existence of the continental slope at that location. The obliqueness of the orientation of the topography step relative to the cross-strait direction is also ignored. These approximations will induce uncertainty in the results for the magnitude of the reflected wave.

Data availability

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Data availability.

The ETOPO1 data (doi: 10.7289/V5C8276M) is available online at https://www.ngdc.noaa.gov/mgg/global/. The DTU10 data is available from ftp://ftp.space.dtu.dk/pub/DTU10.

Competing interests

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Competing interests.

The authors declare that they have no conflict of interest.

Acknowledgements

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Acknowledgements.

This study was supported by the NSFC-Shandong Joint Fund for Marine Science
Research Centers (grant no. U1406404), the National Natural Science
Foundation of China (grant no. 41706031), the Basic Scientific Fund for
National Public Research Institutes of China (grant no. 2014G15), and the
National Key Research and Development Program of China (grant no. 2017YFC1404201).
The authors sincerely thank John M. Huthnance and two anonymous
referees for their constructive comments and suggestions, which are of great
help in improving our study.

Edited by: John M. Huthnance

Reviewed by: two anonymous referees

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Short summary

Taylor's problem is a classical tidal dynamic problem and in its previous applications all of the studied basins had a closed end. In this study, the Taylor's method is extended so that it can also provide an analytical model for the *M*_{2} tide in the Taiwan Strait (TS), which shows that the reflection of the southward wave at the abruptly deepened topography south of the TS is a major contribution to the formation of the northward propagating wave in the strait.

Taylor's problem is a classical tidal dynamic problem and in its previous applications all of...

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